Geometric Algebra for Electrical Engineers., Multivector Electromagnetism., C April 2018 COPYRIGHT

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peeter joot GEOMETRICALGEBRAFORELECTRICALENGINEERS.

GEOMETRICALGEBRAFORELECTRICALENGINEERS.

peeter joot

Multivector Electromagnetism. April 2018 – version V0.1.6 Peeter Joot: Geometric Algebra for Electrical Engineers., Multivector Electromagnetism., c April 2018 COPYRIGHT

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DOCUMENTVERSION

Version V0.1.6 Sources for this notes compilation can be found in the github repository [email protected]:peeterjoot/GAelectrodynamics.git The last commit (Apr/12/2018), associated with this pdf was 725425fef439310c1b62cfb39fd9d3ee389870e3

vii

Dedicated to: Aurora and Lance, my awesome kids, and Soﬁa, who not only tolerates and encourages my studies, but is also awesome enough to think that math is sexy.

PREFACE

This book introduces the fundamentals of geometric algebra and calculus, and applies those tools to the study of electromagnetism. Geometric algebra provides a structure that can represent oriented point, line, plane, and volume segments. Vectors, which can be thought of as a representation of oriented line segments, are generalized to multivectors. A full fledged, but non-commutative (i.e. order matters) multiplication operation will be defined for products of vectors. Namely, the square of a vector is the square of its length. This simple rule, along with a requirement that we can sum vectors and their products, essentially defines geometric algebra. Such sums of scalars, vectors and vector products are called multivectors. The reader will see that familiar concepts such as the dot and cross product are related to a more general vector product, and that algebraic structures such as complex numbers can be represented as multivectors. We will be able to utilize generalized complex exponentials to do rotations in arbitrarily oriented planes in space, and will find that simple geometric algebra representations of many geometric transformations are possible. Generalizations of the divergence and Stokes’ theorems are required once we choose to work with multivector functions. There is an unfortunate learning curve required to express this generalization, but once overcome, we will be left with a single powerful multivector integration theorem that has no analogue in conventional vector calculus. This fundamental theorem of geometric calculus incorporates Green’s (area) theorem, the divergence theorem, Stokes’ theorems, and complex residue calculus. Multivector calculus also provides the opportunity to define a few unique and powerful Green’s functions that almost trivialize solutions of Maxwell’s equations. Instead of working separately with electric and magnetic fields, we will work with a hybrid multivector field that includes both electric and magnetic field contributions, and with a multivector current that includes both charge and current densities. The natural representation of Maxwell’s equations is a single multivector equation that is easier to solve and manipulate then the conventional mess of divergence and curl equations are familiar to the reader. This book is aimed at graduate or advanced undergraduates in electrical engineering or physics. While all the fundamental results of electromagnetism are derived from Maxwell’s equations, there will be no attempt to motivate Maxwell’s equations themselves, so existing familiarity with the subject is desirable.

These notes contain:

• An introduction to Geometric Algebra (GA).

xi • Geometric calculus, and Green’s function solutions of diﬀerential equations.

• Application of Geometric Algebra to electromagnetism.

Prerequisites: It will be assumed that the reader is familiar with rotation matrices, complex numbers, dot and vector products and vector spaces, coordinate representation, linear transformations, determinants, Stokes, Green’s and divergence theorems.

Thanks: I’d like to thank Steven De Keninck, and Dr. Wolfgang Lindner for their review of some of the earlier drafts of this book. Their suggestions signiﬁcantly improved the quality and readability of the text. Peeter Joot [email protected]

xii CONTENTS

Preface xi 1 geometric algebra.1 1.1 Prerequisites.1 1.1.1 Vector space.1 1.1.2 Basis, span and dimension.2 1.1.3 Standard basis, length and normality.3 1.2 Deﬁnitions6 1.2.1 Multivector space.6 1.2.2 Nomenclature. 14 1.3 Colinear vectors. 16 1.4 Normal vectors. 17 1.5 2D multiplication table. 18 1.6 Plane rotations. 20 1.7 Duality. 25 1.8 Vector product, dot product and wedge product. 27 1.9 Reverse. 34 1.10 Complex representations. 35 1.11 Multivector dot product. 37 1.11.1 Dot product of a vector and bivector 39 1.11.2 Bivector dot product. 41 1.11.3 Problems. 42 1.12 Permutation within scalar selection. 42 1.13 Multivector wedge product. 43 1.13.1 Problems. 45 1.14 Projection and rejection. 45 1.15 Normal factorization of the wedge product. 50 1.16 The wedge product as an oriented area. 51 1.17 General rotation. 53 1.18 Symmetric and antisymmetric vector sums. 56 1.19 Reﬂection. 57 1.20 Linear systems. 58 1.21 A summary comparision. 62 1.22 Problem solutions. 64 2 multivector calculus. 65

xiii xiv contents

2.1 Reciprocal frames. 65 2.1.1 Motivation and deﬁnition. 65 2.1.2 R2 reciprocal frame. 69 2.1.3 R3 reciprocal frame. 71 2.1.4 Problems. 72 2.2 Curvilinear coordinates. 73 2.2.1 Two parameters. 73 2.2.2 Three (or more) parameters. 77 2.2.3 Gradient. 77 2.2.4 Vector derivative. 79 2.2.5 Examples. 80 2.2.6 Problems. 89 2.3 Integration theory. 90 2.3.1 Hypervolume integral 90 2.3.2 Fundamental theorem. 91 2.3.3 Stokes’ theorem. 92 2.3.4 Line integral. 93 2.3.5 Surface integral. 96 2.3.6 Two parameter Stokes’ theorem. 99 2.3.7 Green’s theorem. 101 2.3.8 Volume integral. 103 2.3.9 Three parameter Stokes’ theorem. 107 2.3.10 Divergence theorem. 110 2.4 Multivector Fourier transform and phasors. 110 2.5 Green’s functions. 111 2.5.1 Motivation. 111 2.5.2 Green’s function solutions. 115 2.5.3 Helmholtz equation. 117 2.5.4 First order Helmholtz equation. 119 2.5.5 Spacetime gradient. 121 2.6 Helmholtz theorem. 122 2.7 Problem solutions. 126 3 electromagnetism. 129 3.1 Conventional formulation. 129 3.1.1 Problems. 132 3.2 Maxwell’s equation. 132 3.3 Wave equation and continuity. 135 3.4 Plane waves. 137 3.5 Statics. 141 contents xv

3.5.1 Inverting the Maxwell statics equation. 141 3.5.2 Enclosed charge. 143 3.5.3 Enclosed current. 144 3.5.4 Example field calculations. 147 3.6 Dynamics. 160 3.6.1 Inverting Maxwell’s equation. 160 3.7 Energy and momentum. 162 3.7.1 Field energy and momentum density and the energy momentum tensor. 162 3.7.2 Poynting’s theorem (prerequisites.) 167 3.7.3 Poynting theorem. 171 3.7.4 Examples: Some static fields. 174 3.7.5 Complex energy and power. 178 3.8 Lorentz force. 180 3.8.1 Statement. 180 3.8.2 Constant magnetic field. 182 3.9 Polarization. 184 3.9.1 Phasor representation. 184 3.9.2 Transverse plane pseudoscalar. 184 3.9.3 Pseudoscalar imaginary. 190 3.10 Transverse fields in a waveguide. 192 3.11 Multivector potential. 195 3.11.1 Definition. 195 3.11.2 Gauge transformations. 198 3.11.3 Far field. 201 3.12 Dielectric and magnetic media. 204 3.12.1 Statement. 204 3.12.2 Alternative form. 207 3.12.3 Gauge like transformations. 208 3.12.4 Boundary value conditions. 210 a distribution theorems. 213 b proof sketch for the fundamental theorem of geometric calculus. 217 c green’s functions. 221 c.1 Helmholtz operator. 221 c.2 Delta function derivatives. 224 d ga electrodynamics in the literature. 227 e energy momentum tensor for vector parameters. 229 f mathematica notebooks. 231 xvi contents

index 236

bibliography 239 LISTOFFIGURES

Figure 1.1 Vector illustration.7 Figure 1.2 Graphical vector addition.7 Figure 1.3 Unit bivectors for R3 9 Figure 1.4 Circular representation of two bivectors.9 Figure 1.5 Graphical representations of e1e2. 10 Figure 1.6 Graphical representation of bivector addition in plane. 11 Figure 1.7 Bivector addition. 11 Figure 1.8 e1 + e2. 17 Figure 1.9 Multiplication by e1e2. 20 Figure 1.10 π/2 rotation in the plane using pseudoscalar multiplication. 21 Figure 1.11 Rotation in a plane. 22 Figure 1.12 Radial vector in polar coordinates. 23 Figure 1.13 R3 duality illustration. 26 Figure 1.14 Two vectors in a plane. 27 Figure 1.15 Equilateral triangle in R3. 29 Figure 1.16 Projection and rejection illustrated. 46 Figure 1.18 Parallelogram representations of wedge products. 52 Figure 1.19 Different shape representations of a wedge product. 53 Figure 1.20 Rotation with respect to the plane of a pseudoscalar. 56 Figure 1.21 Reflection. 59 Figure 1.22 Intersection of two lines. 61 Figure 1.17 Two equivalent bivector factorizations. 64 Figure 2.1 Oblique and reciprocal bases. 68 Figure 2.2 Contours for an elliptical region. 74 Figure 2.3 Differentials for an elliptical parameterization. 74 Figure 2.4 Two parameter manifold. 76 Figure 2.5 Polar coordinates. 81 Figure 2.6 Toroidal parameterization. 88 Figure 2.7 One parameter manifold. 94 Figure 2.8 Two parameter manifold differentials. 96 Figure 2.9 Contour for two parameter surface boundary. 99 Figure 2.10 Sum of infinitesimal loops. 100 Figure 2.11 Three parameter volume element. 104 Figure 2.12 Differential surface of a volume. 107

xvii xviii List of Figures

Figure 3.1 Line charge density. 147 Figure 3.2 Circular line charge. 153 Figure 3.3 Field due to a circular distribution. 155 Figure 3.4 (a) A(z˜, ρ˜). (b) B(z˜, ρ˜). 157 Figure 3.5 Electric field direction for circular charge density distribution near z = 0. 157 Figure 3.6 Magnetic field direction for circular current density distribution near z = 0. 158 Figure 3.7 Magnetic field for larger z. 158 Figure 3.8 Magnetic field between two current sources. 159 Figure 3.9 Linear polarization. 186 Figure 3.10 Electric field with elliptical polarization. 188 Figure 3.11 Vertical infinitesimal dipole and selected propagation direction. 203 Figure 3.12 Pillbox integration volume. 211 Figure C.1 Neighbourhood kx − x0k < . 222 GEOMETRICALGEBRA. 1

1.1 prerequisites.

Geometric algebra (GA for short), generalizes and extends vector algebra. The following section contains a lighting review of some foundational concepts, including vector space, basis, orthonormality, and metric. If you are inclined to skip this, please at least examine the stated dot product deﬁnition, since the conventional positive deﬁnite property is not assumed.

1.1.1 Vector space.

Vectors have many generalizations in mathematics, where a number of disparate mathematical objects can all be considered vectors. A vector space is an enumeration of the properties and operations that are common to a set of vector-like objects, allowing them to be treated in a uniﬁed fashion, regardless of their representation and application.

Deﬁnition 1.1: Vector space.

A (real) vector space is a set V = {x, y, z, ···}, the elements of which are called vectors, which has an addition operation designated + and a scalar multiplication operation designated by juxtaposition, where the following axioms are satisﬁed for all vectors x, y, z ∈ V and scalars a, b ∈ R

1 2 geometric algebra.

Vector space axioms. Addition is closed. x + y ∈ V (Scalar) multiplication is closed. ax ∈ V Addition is associative. (x + y) + z = x + (y + z) Addition is commutative. y + x = x + y There exists a zero element 0 ∈ V. x + 0 = x For any x ∈ V there exists a negative x + (−x) = 0 additive inverse −x ∈ V. (Scalar) multiplication is distributive. a(x + y) = ax + ay, (a + b)x = ax + bx (Scalar) multiplication is associative. (ab)x = a(bx) There exists a multiplicative identity 1. 1x = x

Despite the generality of this deﬁnition, the vector spaces used in GA are fairly restricted. In particular, electrodynamic applications of GA require only two, three or four dimensional real vector spaces. No vector spaces with matrix, polynomial, or complex tuple elements will be required, nor will any inﬁnite dimensional vector spaces. The only unconventional vector space of interest will be a “space-time” vector space containing a time like “direction”, 1-3 spatial directions, and a generalized length operation that can be negative.

Exercise 1.1 RN N N Define R as the set of tuples {(x1, x2, ···) | xi ∈ R}. Show that R is a vector space when the addition operation is defined as x + y ≡ (x1 + y1, x2 + y2, ···) , and scalar multiplication is N N defined as ax ≡ (ax1, ax2, ···) for any x = (x1, x2, ···) ∈ R , y = (y1, y2, ···) ∈ R , and a ∈ R.

1.1.2 Basis, span and dimension.

Deﬁnition 1.2: Linear combination

Let S = {x1, x2, ··· , xk} be a subset of a vector space V. A linear combination of vectors in S is any sum

a1x1 + a2x2 + ··· + akxk. 1.1 prerequisites. 3

Deﬁnition 1.3: Linear dependence.

Let S = {x1, x2, ··· , xk} be a subset of a vector space V. This set S is linearly dependent if any equation

0 = a1x1 + a2x2 + ··· + akxk,

can be constructed for which not all of the coeﬃcients ai are zero.

Deﬁnition 1.4: Linear independence.

Let S = {x1, x2, ··· , xk} be a subset of a vector space V. This set is linearly independent if there are no equations with ai , 0 such that

0 = a1x1 + a2x2 + ··· + akxk.

Deﬁnition 1.5: Span.

Let S = {x1, x2, ··· , xk} be a subset of a vector space V. The span of this set is the set of all linear combinations of these vectors, denoted

span(S ) = {a1x1 + a2x2 + ··· + akxk} .

Deﬁnition 1.6: Subspace.

Let S = {x1, x2, ··· , xk} be a subset of a vector space V. This subset is a subspace if S is a vector space under the multiplication and addition operations of the vector space V.

Deﬁnition 1.7: Basis and dimension

Let S = {x1, x2, ··· , xn} be a linearly independent subset of V. This set is a basis if span(S ) = V. The number of vectors n in this set is called the dimension of the space.

1.1.3 Standard basis, length and normality. 4 geometric algebra.

Deﬁnition 1.8: Dot product.

Let x, y be vectors from a vector space V. A dot product x · y is a mapping V × V → R with the following properties Dot product properties. Symmetric in both arguments x · y = y · x Bilinear (ax + by) · (a0x0 + b0y0) = aa0(x · x0) + bb0(y · y0) + ab0(x · y0) + ba0(y · x0) (Optional) Positive length x · x > 0, x , 0

Because the dot product is bilinear, it is speciﬁed completely by the dot products of a set of basis elements for the space. For example, given a basis {e1, e2, ··· , eN}, and two vectors XN x = xiei i=1 (1.1) XN y = yiei, i=1 the dot product of the two is

    N  N  X  X  x · y =  xiei ·  y je j     i=1 j=1 (1.2) XN = xiy j ei · e j . i, j=1 Such an expansion in coordinates can be written in matrix form as x · y = xTGy, (1.3)

where G is the symmetric matrix with elements gi j = ei · e j. This matrix G, or its elements gi j is also called the metric for the space. For Euclidean spaces, which are the primary focus of this book, the metric is not only diag- onal, but is the identity matrix. Slightly more general metrics are of interest in electrodynamics. In particular, a four dimensional (relativistic) vector space, where the metric has diagonals (1, −1, −1, −1) or (−1, 1, 1, 1) allows for the construction of a geometric algebra that allows Maxwell’s equations to take their very simplest form. Such a metric does not have the (Eu- clidean) positive deﬁnite property xTGx > 0, x , 0. 1.1 prerequisites. 5

Deﬁnition 1.9: Length

The squared norm of a vector x is deﬁned as

kxk2 = x · x, a quantity that need not be positive. The length of a vector x is deﬁned as p kxk = |x · x|.

Deﬁnition 1.10: Unit vector

A vector x is called a unit vector if its absolute squared norm is one (|x · x| = 1).

Deﬁnition 1.11: Normal

Two vectors from a vector space V are normal, or orthogonal, if their dot product is zero, x · y = 0 ∀x, y ∈ V.

Deﬁnition 1.12: Orthonormal

Two vectors x, y are orthonormal if they are both unit vectors and normal to each other (x · y = 0, |x · x| = |y · y| = 1). A set of vectors {x, y, ··· , z} is an orthonormal set if all pairs of vectors in that set are orthonormal.

Deﬁnition 1.13: Standard basis.

A basis {e1, e2, ··· , eN} is called a standard basis if that set is orthonormal.

Deﬁnition 1.14: Euclidean space. 6 geometric algebra.

A vector space with basis {e1, e2, ··· , eN} is called Euclidean if all the dot product pairs between the basis elements are not only orthonormal, but positive deﬁnite. That is

ei · e j = δi j.

1.2 definitions

1.2.1 Multivector space.

Geometric algebra takes a vector space and adds two additional operations, a vector multiplication operation, and a generalized addition operation that extends vector addition to include addition of scalars and products of vectors. Multiplication of vectors is indicated by juxtaposition, for example, if x, y, e1, e2, e3, ··· are vectors, then some vector products are

xy, xyx, xyxy,

e1e2, e2e1, e2e3, e3e2, e3e1, e1e3, (1.4) e1e2e3, e3e1e2, e2e3e1, e3e2e1, e2e1e3, e1e3e2,

e1e2e3e1, e1e2e3e1e3e2, ···

Vector multiplication is constrained by a rule, called the contraction axiom, that gives a meaning to the square of a vector

xx ≡ x · x. (1.5)

The square of a vector, by this deﬁnition, is the squared length of the vector, and is a scalar. This may not appear to be a useful way to assign meaning to the simplest of vector products, since the product and the vector live in separate spaces. If we want a closed algebraic system that includes both vectors and their products, we have to allow for the addition of scalars, vectors, or any products of vectors. Such a sum is called a multivector, an example of which is

1 + 2e1 + 3e1e2 + 4e1e2e3. (1.6)

In this example, we have added a scalar (or 0-vector) 1, to a vector (or 1-vector) 2e1, to a bivector (or 2-vector) 3e1e2, to a trivector (or 3-vector) 4e1e2e3. Geometric algebra uses vector multiplication to build up a hierarchy of geometrical objects, representing points, lines, planes, volumes and hypervolumes (in higher dimensional spaces.)

Scalar. A scalar, which we will also call a 0-vector, is a zero-dimensional object with sign, and a magnitude. We may geometrically interpret a scalar as a (signed) point in space. 1.2 definitions 7

Vector. A vector, which we will also call a 1-vector, is a one-dimensional object with a sign, a magnitude, and a rotational attitude within the space it is embedded. When vectors are negated the relative placement of the “head” vs. the “tail” are toggled as illustrated in ﬁg. 1.1.

x -x

Figure 1.1: Vector illustration.

Vectors can be added graphically by connecting them head to tail in sequence, and joining the first tail point to the final head, as illustrated in fig. 1.2.

a+b

Figure 1.2: Graphical vector addition.

Bivector. We now wish to deﬁne a bivector, or 2-vector, as a 2 dimensional object representing a signed plane segment with magnitude and orientation. Formally, assuming a vector product, the algebraic description of a bivector is 8 geometric algebra.

Deﬁnition 1.15: Bivector.

A bivector, or 2-vector, is a sum of products of pairs of normal vectors. Given an N dimensional vector space V with an orthonormal basis {e1, e2, ··· , eN}, a general bivector can be expressed as X Bi jeie j, 1≤i< j≤N

where Bi j is a scalar. The vector basis V is said to be a generator of a bivector space.

The bivector provides a structure that can encode plane oriented quantities such as torque, angular momentum, or a general plane of rotation. A quantity like angular momentum can be represented as a magnitude times a quantity that represents the orientation of the plane of rotation. In conventional vector algebra we use the normal of the plane to describe this orientation, but that is problematic in higher dimensional spaces where there is no unique normal. Use of the normal to represent a plane is also logically problematic in two dimensional spaces, which have to be extended to three dimensions to use normal centric constructs like the cross product. A bivector representation of a plane can eliminate the requirement utilize a third (normal) dimension, which may not be relevant in the problem, and can allow some concepts (like the cross product) to be generalized to dimensions other than three when desirable. One of the implications of the contraction axiom eq. (1.5), to be discussed in more detail a bit later, is a linear dependence between bivectors formed from normal products. For example, given any pair of unit bivectors, where i , j we have

eie j + e jei = 0, (1.7)

This is why the sum in definition 1.15 was over only half the possible pairs of i , j indexes. The reader can check that the set of all bivectors is a vector space per definition 1.1, so we will call 2 the set of all bivectors a bivector space. In R a basis for the bivector space is {e1e2}, whereas 3 3 in R a basis for the bivector space is {e1e2, e2e3, e3e1}. The unit bivectors for two possible R bivector space bases are illustrated in fig. 1.3. We interpret the sign of a vector as an indication of the sense of the vector’s “head” vs “tail”. For a bivector, we can interpret the sign as a representation of a a “top” vs. “bottom”, or equivalently a left or right “handedness”, as illustrated using arrows around a plane segment in fig. 1.4. For a product like e1e2, the sense of the handedness follows the path 0 → e1 → e1 + e2 → e2 → 0 around the unit square in the x-y plane. This is illustrated for all the unit bivectors in fig. 1.3. In R3 we can use the right hand rule to visualize such a handedness. You could say that we are using the direction of the fingers around the normal to indicate the sign of the bivector, but without actually drawing that normal. 1.2 definitions 9

(a) (b)

Figure 1.3: Unit bivectors for R3

Figure 1.4: Circular representation of two bivectors. 10 geometric algebra.

Similar to the interpretation of the magnitude of a vector as the length of that vector, we interpret the magnitude of a bivector (to be defined more exactly later), as the area of the bivector. Other than having a boundary that surrounds a given area, a graphical bivector representation as a plane segment need not have any specific geometry, which is illustrated in fig. 1.5 for a set of bivectors all representing e1e2.

Figure 1.5: Graphical representations of e1e2.

An oriented plane segment can always be represented as a bivector in any number of dimensions, however, when the generating vector space has dimension N ≥ 4 not all bivectors defined by definition 1.15 necessarily represent oriented plane segments. The restrictions required for a bivector to have an associated oriented plane segment interpretation in higher dimensional spaces will be defined later. Vector addition can be performed graphically by connecting vectors head to tail, and joining the first tail to the last head. A similar procedure can be used for bivector addition as well, but gets complicated if the bivectors lie in different planes. Here is a simple bivector sum

3e1e2 − 2e1e2 + 5e1e2 = 6e1e2, (1.8)

which can be interpreted as taking a 3 unit area, subtracting a 2 unit area, and adding a 5 unit area. This sum is illustrated in ﬁg. 1.6. An visualization of arbitrarily oriented bivector addition can be found in ﬁg. 1.7, where blue + red = green. This visualization shows that the moral of the story is that we will almost exclusively be adding bivectors algebraically, but can interpret the sum geometrically after the fact.

Trivector. Again, assuming a vector product 1.2 definitions 11

++ =

Figure 1.6: Graphical representation of bivector addition in plane.

Figure 1.7: Bivector addition. 12 geometric algebra.

Deﬁnition 1.16: Trivector.

A trivector, or 3-vector, is a sum of products of triplets of mutually normal vectors. Given an N dimensional vector space V with an orthonormal basis {e1, e2, ··· , eN}, a trivector is any value X Ti jkeie jek, 1≤i< j

where Ti jk is a scalar. The vector space V is said to generate a trivector space.

3 In R all trivectors are scalar multiples of e1e2e3. Like scalars, there is no direction to such a quantity, but like scalars trivectors may be signed. The magnitude of a trivector may be interpreted as a volume. We will defer interpreting the sign of a trivector geometrically until we tackle integration theory.

K-vector.

Deﬁnition 1.17: K-vector and grade.

A k-vector is a sum of products of k mutually normal vectors. Given an N dimensional vector space with an orthonormal basis {e1, e2, ··· , eN}, a general k-vector can be expressed as X Ki j···meie j ··· em, 1≤i< j···

where Ki j···m is a scalar, indexed by k indexes i, j, ··· , m. The number k of normal vectors that generate a k-vector is called the grade. A 1-vector is deﬁned as a vector, and a 0-vector is deﬁned as a scalar. The vector space V is said to generate the k-vector space.

We will see that the highest grade for a k-vector in an N dimensional vector space is N.

Multivector space.

Deﬁnition 1.18: Multivector space.

Given an N dimensional (generating) vector space V with an orthonormal basis {e1, e2, ··· , eN}, and a vector multiplication operation represented by juxtaposition, a multivector is a sum 1.2 definitions 13

P P P of k-vectors, k ∈ [1, N], such as a0 + i aiei + i, j ai jeie j + i, j,k ai jkeie jek + ···, where a0, ai, ai j, ··· are scalars. The multivector space generated by V is a set M = {x, y, z, ···} of multivectors, where the following axioms are satisﬁed Multivector space axioms. Contraction. x2 = x · x, ∀x ∈ V Addition is closed. x + y ∈ M Multiplication is closed. xy ∈ M Addition is associative. (x + y) + z = x + (y + z) Addition is commutative. y + x = x + y There exists a zero element 0 ∈ M. x + 0 = x There exists a negative additive inverse x + (−x) = 0 −x ∈ M. Multiplication is distributive. x(y + z) = xy + xz, (x + y)z = xz + yz Multiplication is associative. (xy)z = x(yz) There exists a multiplicative identity 1. 1x = x

Compared to the vector space, def’n. 1.1, the multivector space

• presumes a vector multiplication operation, which is not assumed to be commutative (order matters),

• generalizes vector addition to multivector addition,

• generalizes scalar multiplication to multivector multiplication (of which scalar multiplication and vector multiplication are special cases),

• and most importantly, speciﬁes a rule providing the meaning of a squared vector (the contraction axiom).

The contraction axiom is arguably the most important of the multivector space axioms, as it allows for multiplicative closure without an inﬁnite dimensional multivector space. The remaining set of non-contraction axioms of a multivector space are almost that of a ﬁeld 1 (as encountered in the study of complex inner products), as they describe most of the properties

1 A mathematician would call a multivector space a non-commutative ring with identity [22], and could state the multivector space deﬁnition much more compactly without listing all the properties of a ring explicitly as done above. 14 geometric algebra.

one would expect of a “well behaved” set of number-like quantities. However, a ﬁeld also requires a multiplicative inverse element for all elements of the space, which exists for some multivector subspaces, but not in general.

1.2.2 Nomenclature.

The workhorse operator of geometric algebra is called grade selection, deﬁned as

Deﬁnition 1.19: Grade selection operator

Given a set of k-vectors Mk, k ∈ [0, N], and any multivector of their sum

XN M = Mi, i=0 the grade selection operator is deﬁned as

hMik ≡ Mk.

Due to its importance, selection of the (scalar) zero grade is given the shorthand

hMi ≡ hMi0 = M0.

The grade selection operator will be used to deﬁne a generalized dot product between multivectors, and the wedge product, which generalizes the cross product (and is related to the cross product in R3). To illustrate grade selection by example, given a multivector M = 3 − e3 + 2e1e2, then

hMi = 3

hMi1 = −e3 (1.9) hMi2 = 2e1e2

hMi3 = 0.

Deﬁnition 1.20: Orthonormal product shorthand. 1.2 definitions 15

Given an orthonormal basis {e1, e2, ···}, a multiple indexed quantity ei j···k should be interpreted as the product (in the same order) of the basis elements with those indexes

ei j···k = eie j ··· ek.

For example,

e12 = e1e2

e123 = e1e2e3 (1.10)

e23121 = e2e3e1e2e1.

Deﬁnition 1.21: Pseudoscalar.

If {x1, x2, ··· , xk} is a normal basis for a k-dimensional (sub)space, then the product x1x2 ··· xk is called a pseudoscalar for that (sub)space. A pseudoscalar that squares to ±1 is called a unit pseudoscalar.

A pseudoscalar is the highest grade k-vector in the algebra, so in R2 any bivector is a pseu- 3 2 doscalar, and in R any trivector is a pseudoscalar. In R , e1e2 is a pseudoscalar, as is 3e2e1, 3 both of which are related by a constant factor. In R the trivector e3e1e2 is a pseudoscalar, as is −7e3e1e2, and both of these can also be related by a constant factor. For the subspace span e1, e2 + e3, one pseudoscalar is e1(e2 + e3). If all the vector factors of a pseudoscalar are not just normal but orthonormal, then it is a unit pseudoscalar. It is conventional to refer to

e12 = e1e2, (1.11) as “the pseudoscalar” for R2, and to

e123 = e1e2e3, (1.12) as “the pseudoscalar” for a three dimensional space. We will see that geometric algebra allows for many quantities that have a complex imaginary nature, and that the pseudoscalars of eq. (1.11) and eq. (1.12) both square to −1. For this reason, it is often convenient to use a imaginary notation for the R2 and R3 pseudoscalars

i = e12 (1.13) I = e123. 16 geometric algebra.

For three dimensional problems in this book, i will often be used as the unit pseudoscalar for whatever planar subspace is relevant to the problem, which may not be the x-y plane. The meaning of i in any such cases will always be deﬁned explicitly.

Exercise 1.2 Permutations of the R3 pseudoscalar Show that all the cyclic permutations of the R3 pseudoscalar are equal

I = e2e3e1 = e3e1e2 = e1e2e3.

Unless otherwise stated, a Euclidean vector space with an orthonormal basis {e1, e2, ···} is assumed for the remainder of this chapter. Generalizations required for non-Euclidean spaces will be discussed when (if?) spacetime vectors are introduced.

1.3 colinear vectors.

It was pointed out that the vector multiplication operation was not assumed to be commutative (order matters). The only condition for which the product of two vectors is order independent, is when those vectors are colinear. Theorem 1.1: Vector commutation.

Given two vectors x, y, if y = αx for some scalar α, then x and y commute

xy = yx.

The proof is simple. yx = αxx (1.14) xy = xαx = αxx. The contraction axiom ensures that the product of two colinear vectors is a scalar. In particular, the square of a unit vector, say u is unity. This should be highlighted explicitly, because this property will be used again and again

u2 = 1. (1.15)

2 2 3 For example, the squares of any orthonormal basis vectors are unity (e1) = (e2) = (e3) = 1. A corollary of eq. (1.15) is that we can factor 1 into the square of any unit vector u

1 = uu. (1.16) 1.4 normal vectors. 17

This factorization trick will be used repeatedly in this book.

1.4 normal vectors.

An interchange of the order of the factors of two normal factors results in a change of sign, for example e2e1 = −e1e2. This is a consequence of the contraction axiom, and can be demonstrated by squaring the vector e1 + e2 (ﬁg. 1.8).

e1 + e2 e2

2 1

Figure 1.8:e 1 + e2.

By the contraction axiom, the square of this vector is 2, so we have

2 2 = (e1 + e2) = (e1 + e2)(e1 + e2) (1.17) 2 2 = e1 + e2 + e2e1 + e1e2. = 2 + e2e1 + e1e2.

We conclude immediately that

e2e1 + e1e2 = 0, (1.18) or

e1e2 = −e1e2. (1.19)

The same computation could have been performed for any two orthonormal vectors, so we conclude that any interchange of two orthonormal vectors changes the sign. In general this is true of any normal vectors. 18 geometric algebra.

Theorem 1.2: Anticommutation

Let u, and v be two normal vectors, the product of which uv is a bivector. Changing the order of these products toggles the sign of the bivector.

uv = −vu.

This sign change on interchange is called anticommutation.

1.52 d multiplication table.

The multiplication table for the R2 geometric algebra can be computed with relative ease. Many of the interesting products involve i = e1e2, the unit pseudoscalar. Using eq. (1.19) the imaginary nature of the pseudoscalar, mentioned early, can now be demonstrated explicitly

2 (e1e2) = (e1e2)(e1e2) = −(e1e2)(e2e1) 2 (1.20) = −e1(e2)e1 2 = −e1 = −1. 1.5 2d multiplication table. 19

Like the (scalar) complex imaginary, this bivector also squares to −1. The only non-trivial products left to ﬁll in the R2 multiplication table are those of the unit vectors with i, products that are order dependent

e1i = e1 (e1e2)

= (e1e1) e2

= e2

ie1 = (e1e2) e1

= (−e2e1) e1

= −e2 (e1e1)

= −e2 (1.21) e2i = e2 (e1e2)

= e2 (−e2e1)

= − (e2e2) e1

= −e1

ie2 = (e1e2) e2

= e1 (e2e2)

= e1.

The multiplication table for the R2 multivector basis can now be tabulated 2D Multiplication table.

1 e1 e2 e1e2

1 1 e1 e2 e1e2

e1 e1 1 e1e2 e2

e2 e2 −e1e2 1 −e1

e1e2 e1e2 −e2 e1 −1 It is important to point out that the pseudoscalar i does not commute with either basis vector, but anticommutes with both, since ie1 = −e1i, and ie2 = −e2i. By superposition i anticommutes with any vector in the x-y plane. More generally, if u and v are orthonormal, and x ∈ span {u, v} then the bivector uv anticommutes with x, or any other vector in this plane. 20 geometric algebra.

1.6 plane rotations.

Plotting eq. (1.21), as in ﬁg. 1.9, shows that multiplication by i rotates the R2 basis vectors by π/2 radians, with the rotation direction dependant on the order of multiplication.

e1(e1e2) e2 1.0 1.0

0.5 0.5

e1 e2(e1e2) (e1e2)e2 -1.0 -0.5 0.5 1.0 -1.0 -0.5 0.5 1.0

-0.5 -0.5

-1.0 -1.0

(e1e2)e1

(a) (b)

Figure 1.9: Multiplication by e1e2.

Using a polar vector representation

x = ρ (e1 cos θ + e2 sin θ) , (1.22)

it can be demonstrated directly that unit pseudoscalar multiplication of an arbitrary vector will induce a π/2 rotation. Multiplying the vector from the right by the pseudoscalar gives

xi = xe1e2 = ρ (e1 cos θ + e2 sin θ) e1e2 (1.23) = ρ (e2 cos θ − e1 sin θ) ,

a counterclockwise rotation of π/2 radians, and multiplying the vector by the pseudoscalar from the left gives

ix = e1e2x = ρe1e2 (e1 cos θ + e2 sin θ) e1e2 (1.24) = ρ (−e2 cos θ + e1 sin θ) ,

a clockwise rotation by π/2 radians (exercise 1.3). 1.6 plane rotations. 21

0 The transformed vector x = xe1e2 = e2e1x(= xi = −ix) has been rotated in the direction that takes e1 to e2, as illustrated in ﬁg. 1.10.

1.0 x(e1e2)

x 0.5

-1.0 -0.5 0.5 1.0

-0.5

-1.0 (e1e2)x

Figure 1.10: π/2 rotation in the plane using pseudoscalar multiplication.

In complex number theory the complex exponential eiθ can be used as a rotation operator. Geometric algebra puts this rotation operator into the vector algebra toolbox, by utilizing Euler’s formula eiθ = cos θ + i sin θ, (1.25) which holds for this pseudoscalar imaginary representation too (exercise 1.4). By writing e2 = e1e1e2, a complex exponential can be factored directly out of the polar vector representation eq. (1.22)

x = ρ (e1 cos θ + e2 sin θ) = ρ (e1 cos θ + (e1e1)e2 sin θ) = ρe1 (cos θ + e1e2 sin θ) (1.26) = ρe1 (cos θ + i sin θ) iθ = ρe1e .

We end up with a complex exponential multivector factor on the right. Alternatively, since e2 = e2e1e1, a complex exponential can be factored out on the left

x = ρ (e1 cos θ + e2 sin θ) = ρ (e1 cos θ + e2(e1e1) sin θ) = ρ (cos θ − e1e2 sin θ) e1 (1.27) = ρ (cos θ − i sin θ) e1 −iθ = ρe e1. 22 geometric algebra.

Left and right exponential expressions have now been found for the polar representation

−iθ iθ ρ (e1 cos θ + e2 sin θ) = ρe e1 = ρe1e . (1.28)

This is essentially a recipe for rotation of a vector in the x-y plane. Such rotations are illustrated in ﬁg. 1.11.

xeiθ 1.0

x 0.5

-1.0 -0.5 0.5 1.0

-0.5 eiθx

-1.0

Figure 1.11: Rotation in a plane.

This generalizes to rotations of RN vectors constrained to a plane. Given orthonormal vectors u, v and any vector in the plane of these two vectors (x ∈ span {u, v}), this vector is rotated θ radians in the direction of rotation that takes u to v by

x0 = xeuvθ = e−uvθx. (1.29)

The sense of rotation for the rotation euvθ is opposite that of evuθ, which provides a ﬁrst hint that bivectors can be characterized as having an orientation, somewhat akin to thinking of a vector as having a head and a tail.

Example 1.1: Velocity and acceleration in polar coordinates.

Complex exponential representations of rotations work very nicely for describing vectors in polar coordinates. A radial vector can be written as r = rrˆ, (1.30)

as illustrated in ﬁg. 1.12. The polar representation of the radial and azimuthal unit vector are simply 1.6 plane rotations. 23

r = r r  θ

r

θ e1

Figure 1.12: Radial vector in polar coordinates.

iθ rˆ = e1e = e1 (cos θ + e1e2 sin θ) = e1 cos θ + e2 sin θ iθ (1.31) θˆ = e2e = e2 (cos θ + e1e2 sin θ) = e2 cos θ − e1 sin θ, where i = e12 is the unit bivector for the x-y plane. We can show that these unit vectors are orthogonal easily

D E rˆ · θˆ = rˆθˆ D iθ −iθ E = e1e e e2 (1.32) = he1e2i = 0, since the scalar grade selection of a bivector is zero. We can ﬁnd the velocity and acceleration by taking time derivatives

v = r0rˆ + rrˆ0 (1.33) a = r00rˆ + 2r0rˆ0 + rrˆ00, but to make these more meaningful want to evaluate the rˆ, θˆ derivatives explicitly. Those are

0 iθ0 iθ 0 iθ 0 rˆ = e1e = e1e1e2e θ = e2e θ = θˆω (1.34) 0 iθ0 iθ 0 iθ 0 θˆ = e2e = e2e1e2e θ = −e1e θ = −rˆω, 24 geometric algebra.

where ω = dθ/dt. The velocity and acceleration vectors can now be written explicitly in terms of radial and azimuthal components. The velocity is

v = r0rˆ + rωθˆ, (1.35)

and the acceleration is

00 0 0 a = r rˆ + 2r ωθˆ + r(ωθˆ) (1.36) = r00rˆ + 2r0ωθˆ + rω0θˆ − rω2rˆ,

or 1 a = rˆ r00 − rω2 + θˆ r2ω 0. (1.37) r Using eq. (1.31), we also have the option of factoring out the rotation operation from the position vector or any of its derivatives

iθ r = (re1) e 0 iθ v = (r e1 + rωe2) e ! (1.38) 1 0 a = r00 − rω2 e + r2ω e eiθ. 1 r 2

In particular, for uniform circular motion, each of the position, velocity and acceleration vectors can be represented by a vector that is ﬁxed in space, subsequently rotated by an angle θ.

Exercise 1.3 R2 rotations. Using familiar methods, such as rotation matrices, show that the counterclockwise and clockwise rotations of eq. (1.22) are given by eq. (1.23) and eq. (1.24) respectively.

Exercise 1.4 Multivector Euler’s formula and trig relations. 1.7 duality. 25

For a multivector x assume an inﬁnite series representation of the exponential, sine and cosine functions and their hyperbolic analogues

∞ X xk ex = k! k=0 ∞ ∞ X x2k X x2k+1 cos x = (−1)k sin x = (−1)k (2k)! (2k + 1)! k=0 k=0 ∞ ∞ X x2k X x2k+1 cosh x = sinh x = (2k)! (2k + 1)! k=0 k=0

a. Show that for scalar θ, and any multivector J that satisﬁes J2 = −1

cosh(Jθ) = cos θ sinh(Jθ) = J sin θ.

b. Show that the trigonometric and hyperbolic Euler formulas

eJθ = cos θ + J sin θ eKθ = cosh θ + K sinh θ,

hold for multivectors J, K satisfying J2 = −1 and K2 = 1 respectively. c. Given multivectors X, Y, show that eX+Y = eXeY if X, Y commute. That is XY = YX.

1.7 duality.

In eq. (1.23) and eq. (1.24) we saw that multiplication by a unit pseudoscalar for a given plane generates normal vectors. For the x-y plane with i = e12, these normal relations can be summarized in polar form as

iθ r = re1e iθ ri = re2e (1.39) iθ ir = −re2e .

Both ir and ri are perpendicular to r with the same magnitude. The direction they point depends on the orientation of the pseudoscalar chosen. For example, had we used an oppositely oriented pseudoscalar i = e2e1, these normal vectors would each have the opposite direction. 26 geometric algebra.

In three dimensions, pseudoscalar multiplication maps bivectors to their normals, or vectors to the bivectors representing the planes that they are normal to. For example, the unit vectors and bivectors are related in the following fashion

e2e3 = Ie1 Ie2e3 = −e1

e3e1 = Ie2 Ie3e1 = −e2 (1.40)

e1e2 = Ie3 Ie1e2 = −e3.

For example, with r = ae1 + be2, we have

rI = (ae1 + be2) e123 = ae23 + be31 (1.41) = e3 (−ae2 + be1) .

Here e3 was factored out of the resulting bivector, leaving two factors both perpendicular to the original vector. Every vector that lies in the span of the plane represented by this bivector is perpendicular to the original vector. This is illustrated in ﬁgure ﬁg. 1.13.

Figure 1.13: R3 duality illustration.

Using pseudoscalar multiplication to produce normal subspaces is referred to as a duality transformation.

Deﬁnition 1.22: Dual

Given a multivector M, the dual of a multivector M is designated M∗ and has the value M∗ = MI, where I is a unit pseudoscalar for the space. 1.8 vector product, dot product and wedge product. 27

Some notes on duality

• If A is a non-scalar k-vector, none of the vector factors of A and A∗ are common.

• In a sense that can be deﬁned more precisely once the general dot product operator is deﬁned, the dual to a given k-vector A represents a (N − k)-vector object that is normal to A.

• The dual of any scalar is a pseudoscalar, whereas the dual of a pseudoscalar is a scalar.

• Some authors use diﬀerent sign conventions for duality, in particular, designating the dual as M∗ = MI−1.

• For non-Euclidean spaces, in particular “null spaces” where the square of vectors can be null, a diﬀerent deﬁnition of duality may be required.

1.8 vector product, dot product and wedge product.

The product of two colinear vectors is a scalar, and the product of two normal vectors is a bivector. The product of two general vectors is a multivector with structure to be determined. A powerful way to examine this structure is to compute the product of two vectors in a polar representation with respect to the plane that they span. Let u and v be an orthonormal pair of vectors in the plane of a and b, oriented in a positive rotational sense as illustrated in ﬁg. 1.14.

Figure 1.14: Two vectors in a plane.

With respect to the orthonormal vectors u and v, a a polar representation of a, b is a = kak ueiabθa = kak e−iabθa u (1.42) b = kbk ueiabθb = kbk e−iabθb u, 28 geometric algebra.

where iab = uv is a unit pseudoscalar for the planar subspace spanned by a and b. The vector product of these two vectors is ab = kak e−iabθa u kbk ueiabθb − = kak kbk e iabθa (uu)eiabθb (1.43) = kak kbk eiab(θb−θa). = kak kbk (cos(θb − θa) + iab sin(θb − θa)) . We see that the product of two vectors is a multivector that has only grades 0 and 2. This can be expressed symbolically as

ab = habi + habi2. (1.44) We recognize the scalar grade of the vector product as the RN dot product, but the grade 2 component of the vector product is something new that requires a name. We respectively identify and deﬁne operators for these vector grade selection operations Deﬁnition 1.23: Dot and wedge products of two vectors.

Given two vectors a, b ∈ RN the dot product is identiﬁed as the scalar grade of their product

habi = a · b.

A wedge product of the vectors is deﬁned as a grade-2 selection operation

a ∧ b ≡ habi2.

Given this notation, the product of two vectors can be written

ab = a · b + a ∧ b.

Scalar grade selection of a product of two vectors is an important new tool. There will be many circumstances where the easiest way to compute a dot product is using scalar grade selection. The split of a vector product into dot and wedge product components is also important. How- ever, to utilize it, the properties of the wedge product have to be determined. Summarizing eq. (1.43) with our new operators, we write

ab = kak kbk exp (iab(θb − θa))

a · b = kak kbk cos(θb − θa) (1.45)

a ∧ b = iab kak kbk sin(θb − θa), 1.8 vector product, dot product and wedge product. 29

Example 1.2: Products of two unit vectors.

To develop some intuition about the vector product, let’s consider product of two unit vectors a, b in the equilateral triangle of ﬁg. 1.15, where 1 a = √ (e3 + e1) = e3 exp (e31π/4) 2 (1.46) 1 b = √ (e3 + e2) = e3 exp (e32π/4) . 2

Figure 1.15: Equilateral triangle in R3.

The product of these vectors is

1 ab = (e + e )(e + e ) 2 3 1 3 2 1 = (1 + e32 + e13 + e12) (1.47) 2 √ 1 3 e + e + e = + 32 √13 12 . 2 2 3 Let the bivector factor be designated e + e + e j = 32 √13 12 . (1.48) 3 30 geometric algebra.

The reader can check (exercise 1.8) that j is a unit bivector (i.e. it squares to −1), allowing us to write √ 1 3 ab = + j 2 2 (1.49) = cos(π/3) + j sin(π/3) = exp ( jπ/3) .

Since both vector factors were unit length, this “complex” exponential has no leading scalar factor contribution from kak kbk. From the above analysis, we can also see that in this case, the product of two 0,2 multivectors was itself a 0,2 multivector. We can see that by forming the product

ab = (exp (−e31π/4) e3)(e3 exp (e32π/4)) (1.50) = exp (−e31π/4) exp (e32π/4) ,

exp (e13π/4) exp (e32π/4) = exp ( jπ/3) . (1.51)

Composition of two rotation operators has resulted in another rotation operator, but that result is in a diﬀerent rotational plane, and through a diﬀerent rotation angle.

Two wedge product properties can be immediately deduced from the polar representation of eq. (1.45)

1. b ∧ a = −a ∧ b.

2. a ∧ (αa) = 0, ∀α ∈ R.

We have now had a few hints that the wedge product might be related to the cross product. Given two vectors a, b both the wedge and the cross product contain a kak kbk sin ∆θ factor, and both the wedge and cross product are antisymmetric operators. The cross product is a bilinear operator (a + b) × (c + d) = a × c + a × c + ···. To see whether this is the case for the wedge product, let’s examine the coordinate expansion of the wedge product. Let X a = aiei i X (1.52) b = biei. i 1.8 vector product, dot product and wedge product. 31

The product of these vectors is

    X  X  ab =  a e   b e   i i  j j i j X = aib jeie j (1.53) i j X X = aib jeie j + aib jeie j. i= j i, j

Since eiei = 1, we see again that the scalar component of the product is the dot product P i aibi. The remaining grade 2 components are the wedge product, for which the coordinate expansion can be simpliﬁed further X a ∧ b = aib jeie j i, j X X = aib jeie j + aib jeie j i< j j

X a a a ∧ b = i j e e . (1.55) i j i< j bi b j

It is now straightforward to show that the wedge product is distributive and bilinear (exercise 1.7). It is also simple to use eq. (1.55) to show that b ∧ a = −a ∧ b and a ∧ a = 0. For R2 there is only one term in eq. (1.55)

a a a ∧ b = 1 2 e e . (1.56) 1 2 b1 b2 We are used to writing the cross product as a 3x3 determinant, which can also be done with the coordinate expansion of the R3 wedge product

e2e3 e3e1 e1e2 X a a a ∧ b = i j e e = . (1.57) i j a1 a2 a3 i j∈{12,13,23} bi b j b1 b2 b3 32 geometric algebra.

Let’s summarize the wedge product properties and relations we have found so far, comparing the R3 wedge product to the cross product Cross product and R3 wedge product comparison. Property Cross product Wedge product Same vectors a × a = 0 a ∧ a = 0 Antisymmetry b × a = −a × b b ∧ a = −a ∧ b Linear a × (αb) = α(a × b) a ∧ (αb) = α(a ∧ b) Distributive a × (b + c) = a × b + a × c a ∧ (b + c) = a ∧ b + a ∧ c

e1 e2 e3 e2e3 e3e1 e1e2

Determinant expansion a × b = a a a a ∧ b = a a a 1 2 3 1 2 3

b1 b2 b3 b1 b2 b3

Polar form nˆ ab kak kbk sin(θb − θa) iab kak kbk sin(θb − θa)

All the wedge properties except the determinant expansion above are valid in any dimension. Comparing eq. (1.57) to the determinant representation of the cross product, and referring to eq. (1.40), shows that the R3 wedge product is related to the cross product by a duality transformation iab = Inˆ ab, or

a ∧ b = I(a × b). (1.58)

The direction of the cross product a × b is normal to the plane represented by the bivector a ∧ b. The magnitude of both (up to a sign) is the area of the parallelogram spanned by the two vectors.

Example 1.3: Wedge and cross product relationship.

To take some of the abstraction from eq. (1.58) let’s consider a speciﬁc example. Let

a = e1 + 2e2 + 3e3 (1.59) b = 4e1 + 5e2 + 6e3.

The reader should check that the cross product of these two vectors is

a × b = −3e1 − 6e2 − 3e3. (1.60) 1.8 vector product, dot product and wedge product. 33

By direct computation, we ﬁnd that the wedge and the cross products are related by a R3 pseudoscalar factor

a ∧ b = (e1 + 2e2 + 3e3) ∧ (4e1 + 5e2 + 6e3) = 5e12 + 6e13 + 8e21 + 12e23 + 12e31 + 15e32 = 3e21 + 6e31 + 3e32 = −3e12 − 6e13 − 3e23 (1.61) = e123(−3e3) + e132(−6e2) + e231(−3e1) = e123(−3e3 − 6e2 − 3e1) = I(a × b).

The relationship between the wedge and cross products allows us to express the R3 vector product as a multivector combination of the dot and cross products

ab = a · b + I(a × b). (1.62)

This is a very important relationship. In particular, for electromagnetism, eq. (1.62) can be used with a = ∇ to combine (the scalar) Gauss’s law with (the vector) Maxwell-Faraday equation, and to combine (the scalar) Gauss’s law for magnetism with (the vector) Ampere-Maxwell equation. Such dot plus cross product sums will yield a pair of multivector equations that can be further merged. The resulting multivector equation will be called Maxwell equation (singular), and will be the starting point of all our electromagnetic analysis.

Exercise 1.5 Wedge product of colinear vectors. Given b = αa, use eq. (1.55) to show that the wedge product of any pair of colinear vectors is zero. Exercise 1.6 Wedge product antisymmetry. Prove that the wedge product is antisymmetric using using eq. (1.55).

Exercise 1.7 Wedge product distributivity and linearity. For vectors a, b, c and d, and scalars α, β use eq. (1.55) to show that a. the wedge product is distributive

(a + b) ∧ (c + d) = a ∧ c + a ∧ d + b ∧ c + b ∧ d, 34 geometric algebra.

b. and show that the wedge product is bilinear

(αa) ∧ (βb) = (αβ)(a ∧ b).

Note that these imply the wedge product also has the cross product ﬁltering property a ∧ (b + αa) = a ∧ b.

Exercise 1.8 Unit bivector. Verify by explicit multiplication that the bivector of eq. (1.48) squares to −1.

1.9 reverse.

Deﬁnition 1.24: Reverse

Let A be a multivector with j multivector factors, A = B1B2 ··· B j, not necessarily normal. The reverse A†, or reversion, of this multivector A is

† † † ··· † A = B j B j−1 B1.

Scalars and vectors are their own reverse, and the reverse of a sum of multivectors is the sum of the reversions of its summands.

Examples:

† (1 + 2e12 + 3e321) = 1 + 2e21 + 3e123 † (1.63) ((1 + e1)(e23 − e12) = (e32 + e12)(1 + e1).

A useful relation for k-vectors that are composed entirely of products of normal vectors exists. We call such k-vectors blades

Deﬁnition 1.25: Blade.

A product of k normal vectors is called a k-blade, or a blade of grade k. A grade zero blade is a scalar. The notation F ∈ Vk is used in the literature to indicate that F is a blade of grade k.

Any k-blade is also a k-vector, but not all k-vectors are k-blades. For example in R4 the bivector

e12 + e34, (1.64) 1.10 complex representations. 35

is not a 2-blade, since it cannot be factored into normal products. This will be relevant when formulating rotations since bivectors that are blades can be used to simply describe rotations or Lorentz boosts 2 whereas it is not easily possible to compute an exponential of a non-blade bivector argument. The reverse of a blade is Theorem 1.3: Reverse of k-blade.

The reverse of a k-blade Ak = a1a2 ··· ak is given by

† k(k−1)/2 Ak = (−1) Ak.

This can be proven by successive interchange of the factors † Ak = akak−1 ··· a1 k−1 = (−1) a1akak−1 ··· a2 k−1 k−2 = (−1) (−1) a1a2akak−1 ··· a3 (1.65) . . k−1 k−2 1 k(k−1)/2 = (−1) (−1) ··· (−1) a1a2 ··· ak, = (−1) a1a2 ··· ak. A special, but important case, is the reverse of the R3 pseudoscalar, which is negated by reversion

I† = −I. (1.66)

1.10 complex representations.

We’ve seen that bivectors like e12 square to minus one. Geometric algebra has inﬁnitely many such imaginary numbers, which can be utilized to introduce problem speciﬁc “complex planes” as desired. In three dimensional and higher spaces, imaginary representations (such as the R3 pseudoscalar) with grades higher than two are also possible. Using the reversion relationship of eq. (1.66), we can see that the I behaves as an imaginary

I2 = I(−I†) = −(e1e2e3)(e3e2e1) (1.67) = −e1e2e2e1 = −e1e1 = −1. 2 A rotation in spacetime. 36 geometric algebra.

Given many possible imaginary representations, complex and complex-like numbers can be represented in GA for any k-vector i that satisﬁes i2 = −1 since the multivector z = x + iy, (1.68)

will have all the required properties of a complex number. For example, in Euclidean spaces we could use either of u ∧ v i = q − (u ∧ v)2 u ∧ v ∧ w (1.69) i = q , − (u ∧ v ∧ w)2

provided u, v(, w) are linearly independent. Given a set of orthonormal vectors u, v(, w), then i = uv (1.70) i = uvw, are also suitable as imaginaries. Other complex number like representations are also possible with GA. Quaternions, which are often used in computer graphics to represent rotations, are the set q ∈ {a + xi + yj + zk | a, x, y, z ∈ R} where

i2 = j2 = k2 = −1 ij = k = −ji (1.71) jk = i = −kj ki = j = −ik.

Like complex numbers, quaternions can be represented in GA as 0,2 multivectors, but require three imaginaries instead of one. Other complex like representations are also possible in GA, provided suitable conjugation operations are defined. For example, an operation called Clifford conjugation (or spatial rever- sal) designated A is introduced in [4] that toggles the sign of any multivector components with grade g mod 4 = 1, 2. Illustrating by example, given a multivector A = 1 + e1 + e12 + e123, the Clifford conjugate is

A = 1 − e1 − e12 + e123, (1.72)

leaving the sign of the scalar and pseudoscalar components untouched (much like the reversion operator † toggles the sign of any grade 2 or 3 multivector components). Such a complex conjugation like operation allows (0,1), (0,2), (1,3) or (2,3) multivectors to encode relativistic “proper length” using geometric algebras built from real Euclidean vector spaces. 1.11 multivector dot product. 37

Exercise 1.9 Quaternions.

Show that the relations eq. (1.71) are satisﬁed by the unit bivectors i = e32, j = e13, k = e21, demonstrating that quaternions, like complex numbers, may be represented as multivector subspaces.

1.11 multivector dot product.

In general the product of two k-vectors is a multivector, with a selection of diﬀerent grades. For example, the product of two bivectors may have grades 0, 2, or 4

e12 (e21 + e23 + e34) = 1 + e13 + e1234. (1.73)

Similarly, the product of a vector and bivector generally has grades 1 and 3

e1 (e12 + e23) = e2 + e123. (1.74)

We’ve identiﬁed the vector dot product with scalar grade selection of their vector product, the selection of the lowest grade of their product. This motivates the deﬁnition of a general multivector dot product

Deﬁnition 1.26: Multivector dot product

PN PN The dot (or inner) product of two multivectors A = i=0 hAii, B = i=0 hBii is deﬁned as

XN D E A · B ≡ A B . i j |i− j| i, j=0

If A, B are k-vectors with equal grade, then the dot product is just the scalar selection of their product A · B = hABi, (1.75) and if A, B are a k-vectors with grades r , s respectively, then their dot product is a single grade selection

A · B = hABi|r−s|. (1.76)

Example 1.4: Multivector dot products. 38 geometric algebra.

The most common and useful multivector dot products are for pairs of multivectors that are each entirely a speciﬁc grade, such as a vector-bivector dot product

· h i (e1 + 2e2) (e12 + e23) = (e1 + 2e2)(e12 + e23) 1 (1.77) = e2 − 2e1 + 2e3,

or a bivector-trivector dot product

· h i (e1 + 2e2) e123 = (e1 + 2e2) e123 2 (1.78) = e23 + 2e31.

Should the products be of mixed grade, then we sum all the individual dot products

(1 + e1 + 2e23) · (e2 − e31) = h1e2i1 + he1e2i + 2he23e2i1 − h1e31i2 − he1e31i1 − 2he23e31i = e2 − 2e3 + e13 + e3. (1.79)

Unfortunately, the notation for the multivector dot product is not standardized. In particular, some authors [7] prefer left and right contraction operations that omit the absolute value in the grade selections. A dot product like operator for scalar selection is also common.

Deﬁnition 1.27: Alternate dot products.

The left and right contraction operations are respectively deﬁned as

XN D E AcB = A B i j j−i i, j=0 XN D E AbB = A B , i j i− j i, j=0

where any selection of a negative grade is taken to be zero. The scalar product is deﬁned as

XN D E A∗B = AiB j i, j=0

In an attempt to avoid inundating the reader with too many new operators, this book will stick to the dot, wedge and grade selection operators. However, these are common enough that they deserve mentioning. 1.11 multivector dot product. 39

1.11.1 Dot product of a vector and bivector

An important example of the generalized dot product is the dot product of a vector and bivector. Unlike the dot product of two vectors, a vector-bivector dot product is order dependent. The vector dot product is zero when the two vectors are normal. This is also true if the vector and bivector are normal, that is, having no common factor, as in

e1 · e23 = he123i1 = 0. (1.80)

On the other hand, a non-zero vector-bivector dot product requires the vector to have some overlap with the bivector. A bivector formed from the product of two normal vectors B = ab, a · b = 0, will have a non-zero dot product with any vector that lies in span {a, b}

(αa + βb) · (ab) = α kak2 b − β kbk2 a. (1.81)

It is often useful to be able to expand a vector-bivector dot product. A useful identity for such an expansion is

Theorem 1.4: Dot product of vector and wedge product.

The dot product of a vector and a wedge product of two vectors distributes as

a · (b ∧ c) = (c ∧ b) · a = (a · b)c − (a · c)b.

Before proving this theorem, let’s take a look at what it implies. This shows that only vectors with some component in the span of the plane represented by the bivector will result in a non- zero vector-bivector dot product. We also know that when a vector that lies entirely in the span of a bivector is multiplied by that bivector, the result is rotated by ±π/2. This means that a vector-bivector dot product is normal to the vector that is dotted with the bivector. This can also be seen algebraically since

a · (a · (b ∧ c)) = a · ((a · b)c − (a · c)b) = (a · c)(a · b) − (a · c)(a · b) (1.82) = 0.

The net eﬀect of a vector-bivector dot product is to select only components of the vector that lie in the plane of the bivector, and then to rotate those by ±π/2 in that plane, plus scale that rotated vector by the magnitude of bivector. 40 geometric algebra.

There are (somewhat tricky) coordinate free ways to prove theorem 1.4 , but a dumber simple expansion in coordinates also does the job. X X D E a · (b ∧ c) = aib jckei · (e j ∧ ek) = aib jck eie jek 1 i, j,k i, j,k X X D E (1.83) (c ∧ b) · a = a b c (e ∧ e ) · e = a b c e e e . i j k k j i i j k k j i 1 i, j,k i, j,k D E If all of i, j, k are unique then e e e = 0, so the vector selection is non-zero only when i i j k 1 equals one of j, k. For example

he1e1e2i1 = e2 (1.84) he1e2e1i1 = −e1.

Given j , k, and i = j or i = k, then it is simple to show (exercise 1.10) that D E D E e e e = e e e , (1.85) i j k 1 k j i 1 so a · (b ∧ c) = (c ∧ b) · a. Additionally (exercise 1.11) D E e e e = e (e · e ) − e (e · e ) . (1.86) i j k 1 k j i j k i Plugging eq. (1.86) back into eq. (1.83) proves the theorem

X a · (b ∧ c) = aib jck ek e j · ei − e j (ek · ei) i, j,k (1.87) = (a · b) c − (a · c) b.

The RHS of eq. (1.87) shows that the vector-bivector dot product has the following relation to the R3 triple cross product

Theorem 1.5: Triple cross product.

For vectors in R3, the dot product of a vector and vector wedge product can be expressed as a triple cross product

a · (b ∧ c) = (b × c) × a.

This can be proven by invoking the well known identity for the triple cross product ([14]) a × (b × c) = (a · c)b − (a · b)c. (1.88) 1.11 multivector dot product. 41

Alternatively, it can be proven directly by applying the identity a ∧ b = I(a × b) to the vector- bivector product, and then selecting the vector grade

a (b ∧ c) = aI (b × c) · × ∧ × = I (a (b c)) + I (a (b c)) (1.89) = I (a · (b × c)) + I2a × (b × c) = I (a · (b × c)) + (b × c) × a.

This multivector has a pseudoscalar (grade 3) component, and a vector component, so selecting the grade one component proves the theorem

a (b ∧ c) 1 = a · (b ∧ c) = (b × c) × a. (1.90)

1.11.2 Bivector dot product.

Being able to compute the generalized dot product of two bivectors will also have a number of applications. When those bivectors are wedge products, there is a useful distribution identity for this dot product.

Theorem 1.6: Dot product distribution over wedge products.

Given two sets of wedge products a ∧ b, and c ∧ d, their dot product is

(a ∧ b) · (c ∧ d) = ((a ∧ b) · c) · d = (b · c)(a · d) − (a · c)(b · d).

To prove this, select the scalar grade of the product (a ∧ b)(c ∧ d)

∧ ∧ ∧ − · (a b)(c d) = (a b)(cd c d) (1.91) = (a ∧ b)cd − (a ∧ b)(c · d).

The second term, a bivector, is not of interest since it will be killed by the scalar selection operation. The remainder can be expanded in grades, ﬁrst making use of the fact that a bivector- vector product has only grade 1 and 3 components

(a ∧ b)c = (a ∧ b) · c + h(a ∧ b)ci3. (1.92) Multiplication of the trivector term by d produces a grade 2,4 multivector which can be ignored. The product of (a ∧ b) · c, a vector, with d is a grade 0,2 multivector, of which only the scalar grade is of interest. That is

∧ · ∧ h ∧ ∧ i (a b) (c d) = (a b)(c d) (1.93) = ((a ∧ b) · c) · d. 42 geometric algebra.

To complete the proof, we apply theorem 1.4

((a ∧ b) · c) · d = (a(b · c) − b(a · c)) · d (1.94) = (a · d)(b · c) − (b · d)(a · c).

In R3, this identity also has a cross product equivalent

Theorem 1.7: Dot products of wedges as cross products.

The dot product of two R3 wedge products can be expressed as cross products

(a ∧ b) · (c ∧ d) = −(a × b) · (c × d).

This follows by scalar grade selection

(a ∧ b) · (c ∧ d) = h(a ∧ b)(c ∧ d)i = hI(a × b)I(c × d)i (1.95) = −(a × b) · (c × d).

1.11.3 Problems.

Exercise 1.10 Index permutation in vector selection. Prove eq. (1.85).

Exercise 1.11 Dot product of unit vector with unit bivector. Prove eq. (1.86).

1.12 permutation within scalar selection.

As scalar selection is at the heart of the generalized dot product, it is worth knowing some of the ways that such a selection operation can be manipulated.

Theorem 1.8: Permutation of multivector products in scalar selection. 1.13 multivector wedge product. 43

The factors within a scalar grade selection of a pair of multivector products may be permuted or may be cyclically permuted

hABi = hBAi hAB ··· YZi = hZAB ··· Yi.

It is suﬃcient to prove just the two multivector permutation case. One simple, but inelegant method, is to ﬁrst expand the pair of multivectors in coordinates. Let X X A = a0 + aiei + ai jei j + ··· i i< j X X (1.96) B = b0 + biei + bi jei j + ··· i i< j

Only the products of equal unit k-vectors ei j, ei jk, ··· can contribute scalar components to the sum, so the scalar selection of the products must have the form

X 2 X 2 hABi = a0b0 + aibiei + ai jbi jei j + ··· (1.97) i i< j

This sum is also clearly equal to hBAi, completing the proof.

1.13 multivector wedge product.

We’ve identiﬁed the vector wedge product of two vectors with the selection of the highest grade of their product. Looking back to the multivector products of eq. (1.73), and eq. (1.74) as motivation, a generalized wedge product can be deﬁned that selects the highest grade terms of a given multivector product

Deﬁnition 1.28: Multivector wedge product.

For the multivectors A, B defined in definition 1.26, the wedge (or outer) product is defined as

XN D E A ∧ B ≡ A B . i j i+ j i, j=0

If A, B are a k-vectors with grades r, s respectively, then their wedge product is a single grade selection

A ∧ B = hABir+s. (1.98) 44 geometric algebra.

The most important example of the generalized wedge is the wedge product of a vector with wedge of two vectors

Theorem 1.9: Wedge of three vectors.

The wedge product of three vectors is associative

(a ∧ b) ∧ c = a ∧ (b ∧ c),

so can be written simply as a ∧ b ∧ c.

The proof follows directly from the deﬁnition

(a ∧ b) ∧ c = h(a ∧ b)ci3 h − · i = (ab a b)c 3 (1.99) = habci3 − (a · b)hci3 = habci3,

where the grade-3 selection of a vector is zero by deﬁnition. Similarly

a ∧ (b ∧ c) = ha(b ∧ c)i3 h − · i = a(bc b c) 3 (1.100) = habci3 − (b · c)hai3 = habci3,

which proves the theorem. It is simple to show that the wedge of three vectors is completely antisymmetric (any interchange of vectors changes the sign), and that cyclic permutation a → b → c → a of the vectors leaves it unchanged (exercise 1.12). These properties are also common to the triple product of R3 vector algebra, a fact that is associated with the fact that there is also a determinant structure to the triple wedge product, which can be shown by direct expansion in coordinates

D E a ∧ b ∧ c = aib jckeie jek X 3 = aib jckeie jek i, j,k (1.101) ai a j ak X = e . bi b j bk i jk i< j

This shows that the R3 wedge of three vectors is triple product times the pseudoscalar

a ∧ b ∧ c = (a · (b × c)) I. (1.102)

Note that the wedge of n vectors is also associative. A full proof is possible by induction, which won’t be done here. Instead, as a hint of how to proceed if desired, consider the coordinate expansion of a trivector wedged with a vector

X D E (a ∧ b ∧ c) ∧ d = aib jckeie jekdlel 4 i, j,k,l X (1.103) = aib jckdleie jekel. i, j,k,l This can be rewritten with any desired grouping ((a ∧ b) ∧ c) ∧ d = (a ∧ b) ∧ (c ∧ d) = a ∧ (b ∧ c ∧ d) = ···. Observe that this can also be put into a determinant form like that of eq. (1.101). Whenever the number of vectors matches the dimension of the underlying vector space, this will be a single determinant of all the coordinates of the vectors multiplied by the unit pseudoscalar for the vector space.

1.13.1 Problems.

Exercise 1.12 Properties of the wedge of three vectors. a. Show that the wedge product of three vectors is completely antisymmetric. b. Show that the wedge product of three vectors a ∧ b ∧ c is invariant with respect to cyclic permutation.

Exercise 1.13 R4 wedge of a non-blade with itself. While the wedge product of a blade with itself is always zero, this is not generally true of the wedge products of arbitrary k-vectors in higher dimensional spaces. To demonstrate this, show that the wedge of the bivector B = e1e2 + e3e4 with itself is non-zero. Why is this bivector not a blade?

1.14 projection and rejection.

Let’s now look at how the dot plus wedge product decomposition of the vector product can be applied to compute vector projection and rejection, which are deﬁned as 46 geometric algebra.

Deﬁnition 1.29: Vector projection and rejection.

Given a vector x and vector u the projection of x onto the direction of u is deﬁned as

Proju(x) = (x · uˆ)uˆ,

where uˆ = u/kuk. The rejection of x by u is deﬁned as the component of x that is normal to u

Reju (x) = x − Proju(x).

An example of projection and rejection with respect to a direction vector u is illustrated in ﬁg. 1.16.

x 3.0

2.5 Reju(x)

2.0 u

1.5

1.0 Proju(x)

0.5

0.0 0 1 2 3 4 Figure 1.16: Projection and rejection illustrated.

Computation of the projective and rejective components of a vector x relative to a direction uˆ requires little more than a multiplication by 1 = uˆuˆ, and some rearrangement

x = xuˆuˆ = (xuˆ) uˆ (1.104) = x · uˆ + x ∧ uˆ uˆ = (x · uˆ) uˆ + (x ∧ uˆ) uˆ.

The vector x is split nicely into its projection and rejective components in a complementary fashion

Proju(x) = (x · uˆ) uˆ (1.105a) 1.14 projection and rejection. 47

Reju (x) = (x ∧ uˆ) uˆ. (1.105b) By construction, (x ∧ uˆ) uˆ must be a vector, despite any appearance of a multivector nature. The utility of this multivector rejection formula is not for hand or computer algebra calculations, where it will generally be faster and simpler to compute x − (x · uˆ)uˆ, than to use eq. (1.105b). Instead this will come in handy as a new abstract algebraic tool. When it is desirable to perform this calculation explicitly, it can be done more eﬃciently using a no-op grade selection operation. In particular, a vector can be written as it’s own grade- 1 selection

x = hxi1, (1.106) so the rejection can be re-expressed using deﬁnition 1.26 as a generalized bivector-vector dot product

Reju (x) = (x ∧ uˆ) uˆ 1 = (x ∧ uˆ) · uˆ. (1.107)

In R3, using theorem 1.5, the rejection operation can also be expressed as a triple cross product

Reju (x) = uˆ × (x × uˆ) . (1.108) To help establish some conﬁdence with these new additions to our toolbox, here are a pair of illustrative examples using eq. (1.105b), and eq. (1.107) respectively.

Example 1.5: An R2 rejection.

Let x = ae1 + be2 and u = e1 for which the wedge is x ∧ uˆ = be2e1. Using eq. (1.105b) the rejection of x by u is

Reju (x) = (x ∧ uˆ) uˆ = (be2e1)e1 (1.109) = be2(e1e1) = be2,

as expected.

This example provides some guidance about what is happening geometrically in eq. (1.105b). The wedge operation produces a pseudoscalar for the plane spanned by {x, u} that is scaled as sin θ where θ is the angle between x and u. When that pseudoscalar is multiplied by uˆ, uˆ is rotated in the plane by π/2 radians towards x, yielding the normal component of the vector x. Here’s a slightly less trivial R3 example 48 geometric algebra.

Example 1.6: An R3 rejection.

√ Let x = ae2 + be3 and uˆ = (e1 + e2)/ 2 for which the wedge product is

e23 e31 e12 1 x ∧ uˆ = √ 0 a b 2 1 1 0 (1.110) 1 = √ (e23(−b) − e31(−b) + e12(−a)) 2 1 = √ (b(e32 + e31) + ae21) . 2 Using eq. (1.107) the rejection of x by u is 1 (x ∧ uˆ) · uˆ = (b(e + e ) + ae ) · (e + e ). (1.111) 2 32 31 21 1 2

Each of these bivector-vector dot products has the form ers · et = hersti1 which is zero whenever the indexes r, s, t are unique, and is a vector whenever one of indexes are repeated (r = t, or s = t). This leaves

1 (x ∧ uˆ) · uˆ = (be3 + ae2 + be3 − ae1) 2 (1.112) a = be + (e − e ). 3 2 2 1

Example 1.7: Velocity and acceleration in polar coordinates.

In eq. (1.35), and eq. (1.36) we found the polar representation of the velocity and acceleration vectors associated with the radial parameterization r(r, θ) = rrˆ(θ). We can alternatively compute the radial and azimuthal components of these vectors in terms of their projective and rejective components

v = vrˆrˆ = v · rˆ + v ∧ rˆrˆ (1.113) a = arˆrˆ = a · rˆ + a ∧ rˆrˆ, 1.14 projection and rejection. 49

so v · rˆ = r0 v ∧ rˆ = rωθˆ ∧ rˆ = ωθˆ ∧ r a · rˆ = r00 − rω2 (1.114) 1 0 a ∧ rˆ = r2ω θˆ ∧ rˆ. r We see that it is natural to introduce angular velocity and acceleration bivectors. These both lie in the θˆ ∧ rˆ plane. Of course, it is also possible to substitute the cross product for the wedge product, but doing so requires the introduction of a normal direction that may not intrinsically be part of the problem (i.e. two dimensional problems).

In the GA literature the projection and rejection operations are usually written using the vector inverse

Deﬁnition 1.30: Vector inverse.

Deﬁne the inverse of a vector x, when it exists, as x x−1 = . kxk2

This inverse satisﬁes x−1x = xx−1 = 1.

The vector inverse may not exist in a non-Euclidean vector space where x2 can be zero for non-zero vectors x. In terms of the vector inverse, the projection and rejection operations with respect to u can be written without any reference to the unit vector uˆ = u/kuk that lies along that vector

1 Proju(x) = (x · u) u (1.115) 1 1 Rej (x) = (x ∧ u) = (x ∧ u) · . u u u 50 geometric algebra.

It was claimed in the deﬁnition of rejection that the rejection is normal to the projection. This can be shown trivially without any use of GA (exercise 1.14). This also follows naturally using the grade selection operator representation of the dot product

Reju (x) · Proju(x) = Reju (x) Proju(x) = h(x ∧ uˆ) uˆ (x · uˆ) uˆi D E = (x · uˆ) (x ∧ uˆ) uˆ 2 (1.116) = (x · uˆ) hx ∧ uˆi = 0.

This is zero because the scalar grade of a wedge product, a bivector, is zero by deﬁnition.

Exercise 1.14 Rejection normality

Prove, without any use of GA, that x − Proju(x) is normal to u, as claimed in deﬁnition 1.29.

Exercise 1.15 Rejection example.

a. Repeat example 1.6 by calculating (x ∧ uˆ)uˆ and show that all the grade three components of this multivector product vanish. b. Explicitly calculate x − (x · uˆ)uˆ and show that this matches eq. (1.112).

1.15 normal factorization of the wedge product.

A general bivector has the form X B = ai jei j, (1.117) i, j

which is not necessarily a blade. On the other hand, a wedge product is always a blade 3

Theorem 1.10: Wedge product normal factorization

The wedge product of any two non-colinear vectors a, b always has a normal (2-blade) factorization

a ∧ b = uv, u · v = 0.

3 In R3 any bivector is also a blade [1] 1.16 the wedge product as an oriented area. 51

This can be proven by construction. Pick u = a and v = Reja (b), then a Reja (b) = a ·Reja (b) + a ∧ Reja (b) ! b · a = a ∧ b − a (1.118) kak2 = a ∧ b, since a ∧ (αa) = 0 for any scalar α. The signiﬁcance of theorem 1.10 is that the square of any wedge product is negative

(uv)2 = (uv)(−vu) = −u(v2)u (1.119) = −|u|2|v|2, which in turn means that exponentials with wedge product arguments can be used as rotation operators.

Exercise 1.16 R3 bivector factorization. 3 Find some normal factorizations for the R bivector e12 + e23 + e31.

1.16 the wedge product as an oriented area.

2 The coordinate representation of the R wedge product (eq. (1.56)) had a single e12 bivector factor, whereas the expansion in coordinates for the general RN wedge product was considerably messier (eq. (1.55)). This diﬀerence can be eliminated by judicious choice of basis. A simpler coordinate representation for the RN wedge product follows by choosing an orthonormal basis for the planar subspace spanned by the wedge vectors. Given vectors a, b, let {uˆ, vˆ} be an orthonormal basis for the plane subspace P = span {a, b}. The coordinate representations of a, b in this basis are a = (a · uˆ)uˆ + (a · vˆ)vˆ (1.120) b = (b · uˆ)uˆ + (b · vˆ)vˆ. The wedge of these vectors is a ∧ b = (a · uˆ)uˆ + (a · vˆ)vˆ ∧ (b · uˆ)uˆ + (b · vˆ)vˆ = (a · uˆ)(b · vˆ) − (a · vˆ)(b · uˆ) uˆvˆ (1.121)

a · uˆ a · vˆ = uˆvˆ. b · uˆ b · vˆ 52 geometric algebra.

We see that this basis allows for the most compact (single term) coordinate representation of the wedge product. If a counterclockwise rotation by π/2 takes uˆ to vˆ the determinant will equal the area of the parallelogram spanned by a and b. Let that area be designated

a · uˆ a · vˆ A = . (1.122) b · uˆ b · vˆ

A given wedge product may have any number of other wedge or normal product representations a ∧ b = (a + βb) ∧ b = a ∧ (b + αa) = (Auˆ) ∧ vˆ = uˆ ∧ (Avˆ) (1.123) vˆ = (αAuˆ) ∧ α vˆ0 = (βAuˆ 0) ∧ β These equivalencies can be thought of as different geometrical representations of the same object. Since the spanned area and relative ordering of the wedged vectors remains constant. Some different parallelogram representations of a wedge products are illustrated in fig. 1.18.

Figure 1.18: Parallelogram representations of wedge products.

As there are many possible normal factorizations for a given wedge product, and also many possible wedge products that produce the same value bivector, we can say that a wedge product 1.17 general rotation. 53 represents an area with a speciﬁc cyclic orientation, but any such area is a valid representation. This is illustrated in ﬁg. 1.19.

Figure 1.19: Diﬀerent shape representations of a wedge product.

Exercise 1.17 Parallelogram area. Show that the area A of the parallelogram spanned by vectors

a = a1e1 + a2e2

b = b1e1 + b2e2, is

a a A = ± 1 2 ,

b1 b2 and that the sign is positive if the rotation angle θ that takes aˆ to bˆ is positive, θ ∈ (0, π).

1.17 general rotation.

Equation (1.21) showed that the R2 pseudoscalar anticommutes with any vector x ∈ R2, xi = −ix, (1.124) and that the sign of the bivector exponential argument must be negated to maintain the value of the vector x ∈ R2 on interchange

xeiθ = e−iθx. (1.125)

The higher dimensional generalization of these results are 54 geometric algebra.

Theorem 1.11: Wedge and exponential commutation and conjugation rules.

Given two non-colinear vectors a, b, let the planar subspace formed by their span be designated S = span {a, b}.

(a) Any vector p ∈ S anticommutes with the wedge product a ∧ b

p(a ∧ b) = −(a ∧ b)p.

(b) Any vector n normal to this plane (n · a = n · b = 0) commutes with this wedge product

n(a ∧ b) = (a ∧ b)n.

(c) Reversing the order of multiplication of a vector p ∈ S with an exponential ea∧b, requires the sign of the exponential argument to be negated

pea∧b = e−a∧bp.

This sign change on interchange will be called conjugation.

(d) Any normal vectors n commute with a such a complex exponential

nea∧b = ea∧bn.

The proof relies on the fact that a normal factorization of the wedge product is possible. If p is one of those factors, then the other is uniquely determined by the multivector equation 1 4 a ∧ b = pq, for which we must have q = x (a ∧ b) ∈ S and p · q = 0 . Then

p(a ∧ b) = p(pq) − = p( qp) (1.126) = −(pq)p = −(a ∧ b)p.

4 The identities required to show that q above has no trivector grades, and to evaluate it explicitly in terms of a, b, x, will be derived later. 1.17 general rotation. 55

Any normal n must also be perpendicular to the factors p, q, with n · p = n · q = 0, so

n(a ∧ b) = n(pq) = (−pn)q = −p(−qn) (1.127) = (pq)n = (a ∧ b)n.

For the complex exponentials, introduce a unit pseudoscalar for the plane i = pˆqˆ satisfying i2 = −1 and a scalar rotation angle θ = (a ∧ b)/i, then for vectors p ∈ S

pea∧b = peiθ = p (cos θ + i sin θ) = (cos θ − i sin θ) p (1.128) = e−iθp = e−a∧bp, and for vectors n normal to S

nea∧b = neiθ = n (cos θ + i sin θ) = (cos θ + i sin θ) n (1.129) = eiθn = ea∧bn, which completes the proof. The point of this somewhat abstract seeming theorem is to prepare for the statement of a general RN rotation, which is

Deﬁnition 1.31: General rotation

Let B = {pˆ, qˆ} be an orthonormal basis for a planar subspace with unit pseudoscalar i = pˆqˆ where i2 = −1. The rotation of a vector x through an angle θ with respect to this plane is

−iθ/2 iθ/2 Rθ(x) = e xe .

Here the rotation sense is that of the π/2 rotation from pˆ to qˆ in the subspace S = span B. 56 geometric algebra.

This statement did not make any mention of a normal direction. Such a normal direction is not unique for dimensions higher than 3, nor deﬁned for two dimensions. Instead the rotational sense is deﬁned by the ordering of the factors in the bivector i. To check that this operation has the desired semantics, let x = xk + x⊥, where xk ∈ S and x⊥ · p = 0 ∀p ∈ S . Then

−iθ/2 iθ/2 Rθ(x) = e xe = e−iθ/2 x + x eiθ/2 k ⊥ (1.130) iθ −iθ/2 iθ/2 = xke + x⊥e e iθ = xke + x⊥. As desired, this rotation operation rotates components of the vector that lie in the planar subspace S by θ, while leaving the normal components of the vector unchanged, as illustrated in ﬁg. 1.20. This is what we can call rotation around a normal in R3.

Figure 1.20: Rotation with respect to the plane of a pseudoscalar.

1.18 symmetric and antisymmetric vector sums. 1.19 reflection. 57

Theorem 1.12: Symmetric and antisymmetric vector products.

1. The dot product of vectors x, y can be written as

1 x · y = (xy + yx) . 2

This sum, including all permutations of the products of x and y is called a completely symmetric sum. A useful variation of this relationship is

yx = 2(x · y) − xy.

2. The wedge product of vectors x, y can be written as

1 x ∧ y = (xy − yx) . 2

This sum, including all permutations of the products x and y, with a sign change for any interchange, is called a completely antisymmetric sum.

These identities highlight the symmetric and antisymmetric nature of the respective dot and wedge products in a coordinate free form, and will be useful in the manipulation of various identities. The proof follows by direct computation after ﬁrst noting that the respect vector products are xy = x · y + x ∧ y (1.131a)

yx = y · x + y ∧ x (1.131b) = x · y − x ∧ y. In eq. (1.131b) the interchange utilized the respective symmetric and antisymmetric nature of the dot and wedge products. Adding and subtracting eq. (1.131) proves the result.

1.19 reflection.

Geometrically the reﬂection of a vector x across a line directed along u is the diﬀerence of the projection and rejection 1 1 x0 = (x · u) − (x ∧ u) u u (1.132) 1 = (x · u − x ∧ u) . u 58 geometric algebra.

Using the symmetric and antisymmetric sum representations of the dot and wedge products from theorem 1.12 the reﬂection can be expressed as vector products 1 1 x0 = (¨xu¨ + ux − ¨xu¨ + ux) , (1.133) 2 u yielding a remarkably simple form in terms of vector products

1 x0 = ux . (1.134) u

As an illustration, here is a sample CliﬀordBasic reﬂection computation

In[1]:= ClearAll[u,x, uu, invu,i,o, proj, rej, ux, uxu] u=4e[1] + 2e[2]; x=3e[1] + 3e[2]; uu= InnerProduct[u,u]; invu=u/ uu; i= InnerProduct[x,u]; o= OuterProduct[x,u]; proj=i invu//N// Simplify rej= GeometricProduct[o, invu] //N// Simplify ux= GeometricProduct[u,x] uxu= GeometricProduct[ux, invu] //N// Simplify

Out[1]= 3.6 e[1] + 1.8 e[2]

Out[2]= -0.6 e[1] + 1.2 e[2]

Out[3]= 18 + 6 e[1,2]

Out[4]= 4.2 e[1] + 0.6 e[2]

the results of which are plotted in ﬁg. 1.21.

1.20 linear systems.

Linear systems can be solved using the wedge product. Illustrating by example, consider the following two variable equation in RN ax + by = c. (1.135)

To solve for x simply wedge with b, and to solve for y wedge with a

(ax + by) ∧ b = c ∧ b (1.136) a ∧ (a¡x + by) = a ∧ c, 1.20 linear systems. 59

x 3.0

2.5 1 (x u) u 2.0 u

1.5 1 -(x u) 1.0 1 u (x·u) u 0.5 1 ux u 0.0 0 1 2 3 4

Figure 1.21: Reﬂection. so, if the system has a solution, it is given by 1 x = c ∧ b ∧ a b (1.137) 1 y = a ∧ c. a ∧ b Higher order systems can be solved in the same fashion, but the equation to be solved must be wedged more times. For example, if the n variable system

a1 x1 + a2 x2 ··· + an xn = b, (1.138) has a solution, it is given by 1 x1 = b ∧ a2 ∧ · · · ∧ an a1 ∧ a2 ∧ · · · ∧ an 1 x2 = a1 ∧ b ∧ · · · ∧ an a1 ∧ a2 ∧ · · · ∧ an (1.139) . . 1 xn = a1 ∧ a2 ∧ · · · ∧ b. a1 ∧ a2 ∧ · · · ∧ an If this system has no solution, then these n-vector ratios will not be scalars. For the solution of xk, the numerator in each case is the denominator wedge product with the ak replaced by the solution vector b. If this sounds like Cramer’s rule, that is because the two are equivalent when the dimension of the vector equals the number of variables in the 60 geometric algebra.

3 linear system. For example, consider the solution for x1 of eq. (1.138) for an R system, with a1 = u, a2 = v, a3 = w

b1 v1 w1

e e e b2 v2 w2 1 2 3

b ∧ v ∧ w b3 v3 w3 x = = , (1.140) 1 u ∧ v ∧ w u1 v1 w1

e e e u2 v2 w2 1 2 3

u3 v3 w3

which is exactly the ratio of determinants found in the Cramer’s rule solution of this problem. We get Cramer’s rule for free due to the antisymmetric structure of the wedge product. Cramer’s rule doesn’t apply to cases where the dimension of the space exceeds the number of variables, but a wedge product solution does not have that restriction. As an example, consider the two variable system eq. (1.135) for vectors in R4 as follows       1 1  1              1 0  2  a =   , b =   , c =   . (1.141) 0 0  0        0 1 −1

Here’s a (Mathematica) computation of the wedge products for the solution 5

In[5]:= ClearAll[a,b,c, iab, aWedgeB, cWedgeB, aWedgeC,x,y] a=e[1] +e[2]; b=e[1] +e[4]; c=e[1] + 2e[2] -e[4];

aWedgeB= OuterProduct[a,b]; cWedgeB= OuterProduct[c,b]; aWedgeC= OuterProduct[a,c];

(* 1/aWedgeB*) iab= aWedgeB/ GeometricProduct[aWedgeB, aWedgeB]; x= GeometricProduct[iab, cWedgeB]; y= GeometricProduct[iab, aWedgeC];

{{a ∧ b=, aWedgeB},{c ∧ b=, cWedgeB},

5 Using the CliﬀordBasic.m geometric algebra module from https://github.com/jlaragonvera/Geometric-Algebra. 1.20 linear systems. 61

{a ∧ c=, aWedgeC},{¨ = ¨x},{ÿ = ¨y} } // Grid

Out[5]= a ∧ b = -e[1,2] + e[1,4] + e[2,4] c ∧ b = -2 e[1,2] + 2 e[1,4] + 2 e[2,4] a ∧ c = e[1,2] - e[1,4] - e[2,4] x = 2 y = -1

which shows that 2a − b = c.

1.20.0.1 Example: intersection of two lines.

As a concrete example, let’s solve the intersection of two lines problem illustrated in ﬁg. 1.22.

b 3 0

b1 2

0 0.0 0.5 1.0 1.5 2.0 2.5 3.0 Figure 1.22: Intersection of two lines.

In parametric form, the lines in this problem are

r1(s) = a0 + s(a1 − a0) (1.142) r2(t) = b0 + t(b1 − b0), so the solution, if it exists, is found at the point satisfying the equality

a0 + s(a1 − a0) = b0 + t(b1 − b0). (1.143)

With

u1 = a1 − a0

u2 = b1 − b0 (1.144)

d = a0 − b0, 62 geometric algebra.

the desired equation to solve is

d + su1 = tu2. (1.145)

As with any linear system, we can solve for s or t by wedging both sides with one of u1 or u2

d ∧ u1 = tu2 ∧ u1 (1.146) d ∧ u2 + su1 ∧ u2 = 0.

2 N In R these equations have a solution if u1 ∧ u2 , 0, and in R these have solutions if the bivectors on each sides of the equations describe the same plane (i.e. the bivectors on each side of eq. (1.146) are related by a scalar factor). Put another way, these have solutions when s and t are scalars with the values u ∧ d s = 2 u ∧ u 1 2 (1.147) u ∧ d t = 1 . u1 ∧ u2

Exercise 1.18 Intersection of a line and plane. Let a line be parameterized by

r(a) = p + aa,

and a plane be parameterized by

r(b, c) = q + bb + cc.

a. State the vector equation to be solved, and its solution for a in terms of a ratio of wedge products. b. State the conditions for which the solution exist in R3 and RN. c. In terms of coordinates in R3 write out the ratio of wedge products as determinants and compare to the Cramer’s rule solution.

1.21 a summary comparision.

Here is a summary that compares various GA expressions with close equivalents in traditional vector (or complex) algebra. 1.21 a summary comparision. 63

Comparison of traditional and geometric algebra identities. Name Geometric algebra Traditional algebra Norm squared x2 x · x complex imaginary e12, e123, ··· i complex number x + e12y x + iy vector products

ab = kak kbk exp (iab∆θ) a · b = kak kbk cos (∆θ) a · b = kak kbk cos (∆θ) a × b = nˆ kak kbk sin (∆θ)

a ∧ b = iab kak kbk sin (∆θ) ,(iabnˆ = e123). wedge/cross product anti- a ∧ b = −b ∧ a a × b = −b × a symmetry wedge/cross ﬁltering a ∧ (αa + b) = a ∧ b a × (αa + b) = a × b

P ai a j P ai a j wedge/cross coordinate ex- a ∧ b = i< j eie j a × b = i< j ei × e j pansion bi b j bi b j

e2e3 e3e1 e1e2 e1 e2 e3 wedge/cross determinant a ∧ b = a a a a × b = a a a 1 2 3 1 2 3 expansion b1 b2 b3 b1 b2 b3 vector-bivector dot product a · (b ∧ c) (b × c) × a ( triple cross product) bivector dot product (dot (a ∧ b) · (c ∧ d) −(a × b) · (c × d) product of cross products)

ai a j ak ai a j ak

Triple wedge (triple prod- a ∧ b ∧ c = b b b I a · (b × c) = b b b i j k i j k uct) ci c j ck ci c j ck Normal to vectors a, b I(a ∧ b) a × b Plane normal to a vector n (In) ∧ x = 0 n · x = 0 Plane normal to vectors (a ∧ b) ∧ x = 0 (a × b) · x = 0 a, b Projection (x · uˆ)uˆ (x · uˆ)uˆ Rejection (x ∧ uˆ)uˆ (uˆ × x) × uˆ      cos θ sin θ x iθ     2D rotation xe , i = e12     − sin θ cos θ y 3D rotation in the plane of e−uˆvˆθ/2xeuˆvˆθ/2 (x · uˆ)(uˆ cos θ + vˆ sin θ) + uˆ, vˆ, where uˆ · vˆ = 0 (x · vˆ)(vˆ cos θ − uˆ sin θ) + (uˆ × x) × uˆ Reﬂection uxˆ uˆ (x · uˆ)uˆ + uˆ × (uˆ × x) 64 geometric algebra.

1.22 problem solutions.

Answer for Exercise 1.16 e − e e + e + e = (e + e − 2e ) 2 1 12 23 31 1 2 3 2 e − e = 3 2 (2e − e − e ) . 2 1 2 3 The respective parallelogram representations of these bivector factorizations are illustrated in ﬁg. 1.17, showing the bivectors face on, and from a side view that shows they are coplanar.

(a) (b)

Figure 1.17: Two equivalent bivector factorizations. MULTIVECTORCALCULUS. 2

2.1 reciprocal frames.

2.1.1 Motivation and deﬁnition.

The end goal of this chapter is to be able to integrate multivector functions along curves and surfaces, known collectively as manifolds. For our purposes, a manifold is deﬁned by a parameterization, such as the vector valued function x(a, b) where a, b are scalar parameters. With one parameter the vector traces out a curve, with two a surface, three a volume, and so forth. The respective partial derivatives of such a parameterized vector deﬁne a local basis for the surface at the point at which the partials are evaluated. The span of such a basis is called the tangent space, and the partials that constitute it are not necessarily orthonormal, or even normal. Unfortunately, in order to work with the curvilinear non-orthonormal bases that will be encountered in general integration theory, some additional tools are required.

• We introduce a reciprocal frame which partially generalizes the notion of normal to non- orthonormal bases.

• We will borrow the upper and lower index (tensor) notation from relativistic physics that is useful for the intrinsically non-orthonormal spaces encountered in that study, as this notation works well to deﬁne the reciprocal frame.

Deﬁnition 2.1: Reciprocal frame

Given a basis for a subspace {x , x , ··· x }, not necessarily orthonormal, the reciprocal 1 2n n o frame is deﬁned as the set of vectors x1, x2, ··· xn satisfying

j j xi · x = δi ,

where the vector x j is not the j-th power of x, but is a superscript index, the conventional j way of denoting a reciprocal frame vector, and δi is the Kronecker delta.

Note that any orthonormal basis is also its reciprocal basis. The deﬁnition above introduces mixed index variables for the ﬁrst time in this text, which may be unfamiliar. These are most often used in tensor algebra, where any expression that

65 66 multivector calculus.

has pairs of upper and lower indexes implies a sum, and is called the summation (or Einstein) convention. For example:

i X i aib ≡ aib i (2.1) i j X i j A jBiC ≡ A jBiC . i, j Summation convention will not be used explicitly in this text, as it deviates from normal practises in electrical engineering1.

2.1.1.1 Vector coordinates.

The most important application of a reciprocal frame is for the computation of the coordinates of a vector with respect to a non-orthonormal frame. Let a vector a have coordinates ai with respect to a basis {xi}

X j a = a x j, (2.2) j

where j in a j is an index not a power2. Dotting with the reciprocal frame vectors xi provides these coordinates ai   X  a · xi =  a jx  · xi  j j (2.3) X j i = a δ j j = ai.

The vector can also be expressed with coordinates taken with respect to the reciprocal frame. Let those coordinates be ai, so that

X i a = aix . (2.4) i

1 Generally, when summation convention is used, explicit summation is only used explicitly when upper and lower indexes are not perfectly matched, but summation is still implied. Readers of texts that use summation convention can check for proper matching of upper and lower indexes to ensure that the expressions make sense. Such matching is the reason a mixed index Kronecker delta has been used in the deﬁnition of the reciprocal frame. 2 In tensor algebra, any index that is found in matched upper and lower index pairs, is known as a dummy summation j index, whereas an index that is unmatched is known as a free index. For example, in a bi j (summation implied) j is a summation index, and i is a free index. We are free to make a change of variables of any summation index, so for k the same example we can write a bik. These index tracking conventions are obvious when summation symbols are included explicitly, as we will do. 2.1 reciprocal frames. 67

Dotting with the basis vectors xi provides the reciprocal frame relative coordinates ai

  X  a · x =  a x j · x i  j  i j (2.5) X j = a jδ i j = ai.

We can summarize eq. (2.3) and eq. (2.5) by stating that a vector can be expressed in terms of coordinates relative to either the original or reciprocal basis as follows

X j X j a = a · x x j = (a · x j) x . (2.6) j j

In tensor algebra the basis is generally implied3. An example of a 2D oblique Euclidean basis and a corresponding reciprocal basis is plotted in ﬁg. 2.1. Also plotted are the superposition of the projections required to arrive at a given 1 2 point (4, 2)) along the e1, e2 directions or the e , e directions. In this plot, neither of the re- i ciprocal frame vectors e are normal to the corresponding basis vectors ei. When one of ei is increased(decreased) in magnitude, there will be a corresponding decrease(increase) in the magnitude of ei, but if the orientation is remained ﬁxed, the corresponding direction of the reciprocal frame vector stays the same.

2.1.1.2 Bivector coordinates.

Higher grade multivector objects may also be represented in curvilinear coordinates. Illustrating by example, we will calculate the coordinates of a bivector constrained to a three parameter manifold span {x1, x2, x3} which can be represented as 1 X X B = Bi jx ∧ x = Bi jx ∧ x . (2.7) 2 i j i j i, j i< j

3 In tensor algebra, a vector, identiﬁed by the coordinates ai is called a contravariant vector. When that vector is identiﬁed by the coordinates ai it is called a covariant vector. These labels relate to how the coordinates transform with respect to norm preserving transformations. We have no need of this nomenclature, since we never transform coordinates in isolation, but will always transform the coordinates along with their associated basis vectors. 68 multivector calculus.

x 8 2

2 x 4 (a·x )x2 2 1 2 x (a·x )x1 x 1 a 2 x 1 x1 0

x1 2 2 - (a·x2)x

1 (a·x1)x -4 x2

-6 0 2 4 6 8 10 12

Figure 2.1: Oblique and reciprocal bases. 2.1 reciprocal frames. 69

The coordinates Bi j can be determined by dotting B with x j ∧ xi, where i , j, yielding

j i 1 X rs j i B · x ∧ x = B (xr ∧ xs) · x ∧ x 2 r,s 1 X rs j i = B (xr ∧ xs) · x · x 2 r,s 1 X rs j j i = B xrδs − xsδr · x (2.8) 2 r,s 1 X rs i j i j = B δr δs − δs δr 2 r,s 1 = Bi j − B ji . 2 We see that the coordinates of a bivector, even with respect to a non-orthonormal basis, are antisymmetric, so eq. (2.8) is just Bi j as claimed. That is Bi j = B · x j ∧ xi . (2.9)

Just as the reciprocal frame was instrumental for computation of the coordinates of a vector with respect to an arbitrary (i.e. non-orthonormal frame), we use the reciprocal frame to calculate the coordinates of a bivector, and could do the same for higher grade k-vectors as well.

2.1.2 R2 reciprocal frame.

How are the reciprocal frame vectors computed? While these vectors have a natural GA representation, this is not intrinsically a GA problem, and can be solved with standard linear algebra, using a matrix inversion. For example, given a 2D basis {x1, x2}, the reciprocal basis can be assumed to have a coordinate representation in the original basis

1 x = ax1 + bx2 2 (2.10) x = cx1 + dx2.

Imposing the constraints of deﬁnition 2.1 leads to a pair of 2x2 linear systems that are easily solved to ﬁnd

1 1 2 x = (x2) x1 − (x1 · x2) x2 (x )2(x )2 − (x · x )2 1 2 1 2 (2.11) 2 1 2 x = (x1) x2 − (x1 · x2) x1 . 2 2 2 (x1) (x2) − (x1 · x2) 70 multivector calculus.

The reader may notice that for R3 the denominator is related to the norm of the cross product x1 × x2. More generally, this can be expressed as the square of the bivector x1 ∧ x2

2 − (x1 ∧ x2) = − (x1 ∧ x2) · (x1 ∧ x2) (2.12) = − ((x1 ∧ x2) · x1) · x2 2 2 2 = (x1) (x2) − (x1 · x2) .

Additionally, the numerators are each dot products of x1, x2 with that same bivector x · (x ∧ x ) x1 = 2 1 2 (x ∧ x )2 1 2 (2.13) x · (x ∧ x ) x2 = 1 2 1 , 2 (x1 ∧ x2) or

1 x1 = x · 2 x ∧ x 1 2 (2.14) 2 1 x = x1 · . x2 ∧ x1

Recall that dotting with the unit bivector of a plane (or its inverse) rotates a vector in that plane by π/2. In a plane subspace, such a rotation is exactly the transformation to ensure that 2 1 x1 · x = x2 · x = 0. This shows that the reciprocal frame for the basis of a two dimensional subspace is found by a duality transformation of each of the curvilinear coordinates, plus a subsequent scaling operation. As x1 ∧ x2, the pseudoscalar for the subspace spanned by {x1, x2}, is not generally a unit bivector, the dot product with its inverse also has a scaling eﬀect.

Numerical example: Here is a Mathematica calculation of the reciprocal frame depicted in ﬁg. 2.1

In[6]:= ClearAll[x1, x2, inverse] x1=e[1] +e[2]; x2=e[1] + 2e[2]; x12= OuterProduct[x1, x2]; inverse[a_] := a / GeometricProduct[a, a]; x12inverse= inverse[x12]; s1= InnerProduct[x2, x12inverse]; s2= InnerProduct[x1,-x12inverse]; s1 s2 dots[a_,b_] := {a ," ·", b,"=", InnerProduct[a // ReleaseHold, b // ReleaseHold]}; 2.1 reciprocal frames. 71

MapThread[dots, {{x1// HoldForm, x2// HoldForm, x1// HoldForm, x2// HoldForm}, {s1// HoldForm, s1// HoldForm, s2// HoldForm, s2// HoldForm}}] // Grid

Out[6]= 2 e[1] - e[2]

Out[7]= -e[1] + e[2]

Out[8]= x1 · s1 = 1 x2 · s1 = 0 x1 · s2 = 0 x2 · s2 = 1

This shows the reciprocal vector calculations using eq. (2.14) and that the deﬁning property j j xi · x = δi of the reciprocal frame vectors is satisﬁed.

2 2 Example: R : Given a pair of arbitrary oriented vectors in R , x1 = a1e1 + a2e2, x2 = b1e1 + b2e2, the pseudoscalar associated with the basis {x1, x2} is

∧ ∧ x1 x2 = (a1e1 + a2e2) (b1e1 + b2e2) (2.15) = (a1b2 − a2b1) e12.

The inverse of this pseudoscalar is 1 1 = e21. (2.16) x1 ∧ x2 a1b2 − a2b1 So for this ﬁxed oblique R2 basis, the reciprocal frame is just e x1 = x 21 2 a b − a b 1 2 2 1 (2.17) 2 e12 x = x1 . a1b2 − a2b1

1 The vector x is obtained by rotating x2 by −π/2, and rescaling it by the area of the parallel- 2 ogram spanned by x1, x2. The vector x is obtained with the same scaling plus a rotation of x1 by π/2.

2.1.3 R3 reciprocal frame.

In this section we generalize eq. (2.14) to R3 vectors, which will illustrate the general case by example. 72 multivector calculus.

Given a subspace spanned by a three vector basis {x1, x2, x3} the reciprocal frame vectors can be written as dot products

1 3 2 1 x = (x2 ∧ x3) · x ∧ x ∧ x 2 1 3 2 x = (x3 ∧ x1) · x ∧ x ∧ x (2.18) 3 2 1 3 x = (x1 ∧ x2) · x ∧ x ∧ x .

Each of those trivector terms equals −x1 ∧ x2 ∧ x3 and can be related to the (known) pseudoscalar x1 ∧ x2 ∧ x3 by observing that

 1 2 3 x ∧ x ∧ x · (x3 ∧ x2 ∧ x1) 1 2 3 = x · x · x · (x3 ∧ x2 ∧ x1) 1 2 (2.19) = x · x · (x2 ∧ x1) 1 = x · x1 = 1,

which means that

1 −x1 ∧ x2 ∧ x3 = − x3 ∧ x2 ∧ x1 (2.20) 1 = , x1 ∧ x2 ∧ x3 and

1 1 x = (x2 ∧ x3) · x1 ∧ x2 ∧ x3 2 1 x = (x3 ∧ x1) · (2.21) x1 ∧ x2 ∧ x3 3 1 x = (x1 ∧ x2) · x1 ∧ x2 ∧ x3

Geometrically, dotting with this trivector is a duality transformation within the subspace j j spanned by the three vectors x1, x2, x3, also scaling the result so that the xi · x = δi condition is satisﬁed. The scaling factor is the volume of the parallelepiped spanned by x1, x2, x3.

2.1.4 Problems. 2.2 curvilinear coordinates. 73

Exercise 2.1 Reciprocal frame for two dimensional subspace. Prove eq. (2.11).

Exercise 2.2 Two vector reciprocal frame 3 Calculate the reciprocal frame for the R subspace spanned by {x1, x2} where

x1 = e1 + 2e2 (2.25) x2 = e2 − e3.

2.2 curvilinear coordinates.

2.2.1 Two parameters.

Curvilinear coordinates can be deﬁned for any subspace spanned by a parameterized vector into that space. As an example, consider a two parameter planar subspace of parameterized by the following continuous vector function √ 3 x(u , u ) = u e cosh (atanh(1/2) + e u ) , (2.31) 1 2 1 1 2 12 2

where u1 ∈ [0, 1] and u2 ∈ [0, π/2]. This parameterization spans the first quadrant of the ellipse with semi-major axis length 1, and semi-minor axis length 1/2 4 Contours for this parameterization are plotted in fig. 2.2. The radial contours are for fixed values of u2 and the elliptical contours fix the value of u1, and depict a set of elliptic curves with a semi-major/major axis ratio of 1/2. We define a curvilinear basis associated with each point in the region by the partials ∂x x = 1 ∂u 1 (2.32) ∂x x2 = . ∂u2 For our the function eq. (2.31) our curvilinear basis elements are √ 3 x1 = e1 cosh (atanh(1/2) + e12u2) 2 √ (2.33) 3 x = u e sinh (atanh(1/2) + e u ) . 2 1 2 2 12 2 4 A parameterization of an elliptic area may or may not not be of much use in electrodynamics. It does, however, provide a fairly simple but non-trivial example of a non-orthonormal parameterization. 74 multivector calculus.

0.5

0.4

0.3

0.2

0.1

0.0 0.0 0.2 0.4 0.6 0.8 1.0 Figure 2.2: Contours for an elliptical region.

We form vector valued diﬀerentials for each parameter

dx1 = x1du1 (2.34) dx2 = x2du2.

For eq. (2.31), the values of these diﬀerentials dx1, dx2 with du1 = du2 = 0.1 are plotted in ﬁg. 2.3 for the points (u1, u2) = (0.7, 5π/20), (0.9, 3π/20), (1.0, 5π/20) in (dark-thick) red, blue and purple respectively.

0.5

x2 x1 0.4

x2 x1

x2 x1 0.3 x2 x x1 2 x1 x2 x1 0.2

0.1 0.4 0.5 0.6 0.7 0.8 0.9 Figure 2.3: Diﬀerentials for an elliptical parameterization.

In this case and in general there is no reason to presume that there is any orthonormality constraint on the basis {x1, x2} for a given two parameter subspace. 2.2 curvilinear coordinates. 75

Should we wish to calculate the reciprocal frame for eq. (2.31) , we would find (exercise 2.3) that √ 1 x = e1 3 sinh (atanh(1/2) + e12u2) √ 2 e2 (2.35) x = 3 cosh (atanh(1/2) + e12u2) . u1 These are plotted (scaled by da = 0.1 so they fit in the image nicely) in fig. 2.3 using thin light arrows. When evaluating surface integrals, we will form oriented (bivector) area elements from the wedge product of the differentials

2 d x ≡ dx1 ∧ dx2. (2.36) p This absolute value of this area element −(d2x)2 is the area of the parallelogram spanned by dx1, dx2. In this example, all such area elements lie in the x − y plane, but that need not be the case. Also note that we will only perform integrals for those parametrizations for which the area element d2x is non-zero. Exercise 2.3 Elliptic curvilinear and reciprocal basis. From eq. (2.31), compute the curvilinear coordinates eq. (2.33), and the reciprocal frame vec- i i tors eq. (2.35). Check using scalar grade selection that x · x j = δ j. Hints: Given µ = atanh(1/2),

• cosh(µ + iθ)e2 = e2 cosh(µ − iθ).

• Re (cosh(µ − iθ) sinh(µ + iθ)) = 2/3.

fixme: don’t introduce the idea of tangent space until a 3D example. Remove the R3 reference above, and keep this first example planar. At the point of evaluation, the span of these differentials is called the tangent space. In this particular case the tangent space at all points in the region is the entire x-y plane. These partials locally span the tangent space at a given point on the surface.

2.2.1.1 Curved two parameter surfaces.

Continuing to illustrate by example, let’s now consider a non-planar two parameter surface

2 2 x(u1, u2) = (u1 − u2) e1 + (1 − (u2) )e2 + u1u2e3. (2.37) 76 multivector calculus.

The curvilinear basis elements, and the area element, are

x1 = 2(u1 − u2)e1 + u2e3

x2 = 2(u2 − u1)e1 − 2u2e2 + u1e3 (2.38) 2 2 2 x1 ∧ x2 = −4v1 (u1 − v1) e12 + 2v1e23 + 2v1 − 2u1 e31. Two examples of these vectors and the associated area element (rescaled to ﬁt) is plotted in ﬁg. 2.4. This plane is called the tangent space at the point in question, and has been evaluated at (u1, u2) = (0.5, 0.5), (0.35, 0.75).

Figure 2.4: Two parameter manifold.

The results of eq. (2.38) can be calculated easily by hand for this particular parameterization, but also submit to symbolic calculation software. Here’s a complete example using CliﬀordBa- sic

In[9]:= << CliffordBasic‘; $SetSignature={3,0};

In[10]:= ClearAll[xp,x, x1, x2] (* Use dummy parameter values for the derivatives, and then switch them to function parameter values.*) xp := (a-b)^2e[1] + (1 -b^2)e[2] +bae[3]; x[u_, v_] := xp/.{a → u,b →v}; x1[u_, v_] :=D[xp,a] /. {a → u,b →v}; x2[u_, v_] :=D[xp,b] /. {a → u,b →v};

x1[u,v] x2[u,v] OuterProduct[x1[u,v], x2[u,v]] // GFactor 2.2 curvilinear coordinates. 77

Out[10]= 2 (u-v) e[1] + v e[3]

Out[11]= -2 (u - v) e[1] - 2 v e[2] + u e[3] 2 2 2 2 Out[12]= (-4 u v + 4 v ) e[1,2] + (2 u - 2 v ) e[1,3] + 2 v e[2,3]

2.2.2 Three (or more) parameters.

We can extend the previous two parameter subspace ideas to higher dimensional (or one dimensional) subspaces associated with a parameterization

Deﬁnition 2.2: Curvilinear coordinates and volume element

Given a parameterization x(u1, u2, ··· , uk) with k degrees of freedom, we deﬁne the curvilinear basis elements xi by the partials ∂x xi = . ∂ui

The span of {xi} at the point of evaluation is called the tangent space. A subspace associated with a parameterization of this sort is also called a manifold. The volume element for the subspace is

k d x = du1du2 ··· duk x1 ∧ x2 ∧ · · · ∧ xk.

Such a volume element is a k-vector. The volume of the hyper-parallelepiped bounded by q k 2 {xi} is (d x) .

We will assume that the parameterization is non-generate. This means that the volume element dkx is non-zero in the region of interest. Note that a zero volume element implies a linear dependency in the curvilinear basis elements xi. Given a parameterization x = x(u, v, ··· , w), we may also write xu, xv, ··· , xw for the curvilinear basis elements, and xu, xv, ··· , xw for the reciprocal frame. When doing so, sums over P i numeric indexes like i x xi should be interpreted as a sum over all the parameter labels, i.e. u v x xu + x xv + ···.

2.2.3 Gradient.

With the introduction of the ideas of reciprocal frame and curvilinear coordinates, we are getting closer to be able to formulate the geometric algebra generalizations of vector calculus. 78 multivector calculus.

The next step in the required mathematical preliminaries for geometric calculus is to determine the form of the gradient with respect to curvilinear coordinates and the parameters associated with those coordinates. Suppose we have a vector parameterization of RN

x = x(u1, u2, ··· , uN). (2.39)

We can employ the chain rule to express the gradient in terms of derivatives with respect to ui

X ∂ ∇ = e i ∂x i i X ∂u j ∂ = e i ∂x ∂u i, j i j   (2.40) X X ∂u j  ∂ =  e   i ∂x  ∂u j i i j X ∂ = ∇u . j ∂u j j

It turns out that the gradients of the parameters are in fact the reciprocal frame vectors

Theorem 2.1: Reciprocal frame vectors

Given a curvilinear basis with elements xi = ∂x/∂ui, the reciprocal frame vectors are given by

i x = ∇ui. 2.2 curvilinear coordinates. 79

This can be proven by direct computation

i ∂x x · x j = (∇ui) · ∂u j n ! ! X ∂u ∂x = e i · e s r ∂x s ∂u r,s=1 r j Xn ∂u ∂x = (e · e ) i s r s ∂x ∂u r,s=1 r j Xn ∂u ∂x (2.41) = δ i s rs ∂x ∂u r,s=1 r j Xn ∂u ∂x = i r ∂x ∂u r=1 r j ∂u j = ∂ui = δi j.

i This shows that x = ∇ui has the properties required of the reciprocal frame, proving the theorem. We are now able to deﬁne the gradient with respect to an arbitrary set of parameters

Theorem 2.2: Curvilinear representation of the gradient

N Given an N-parameter vector parameterization x = x(u1, u2, ··· , uN) of R , with curvilinear basis elements xi = ∂x/∂ui, the gradient is X ∂ ∇ = xi . ∂u i i

It is convenient to deﬁne ∂i ≡ ∂/∂ui, so that the gradient can be expressed in mixed index representation

X i ∇ = x ∂i. i

2.2.4 Vector derivative.

Given curvilinear coordinates defined on a subspace definition 2.2, we don’t have enough parameters to define the gradient. For calculus on the k-dimensional subspace, we define the vector derivative 80 multivector calculus.

Deﬁnition 2.3: Vector derivative

N Given a k-parameter vector parameterization x = x(u1, u2, ··· , uk) of R with k ≤ N, and curvilinear basis elements xi = ∂x/∂ui, the vector derivative ∂ is deﬁned as

k X i ∂ = x ∂i. i=1

When the dimension of the subspace (number of parameters) equals the dimension of the underlying vector space, the vector derivative equals the gradient. Otherwise we can write

∇ = ∂ + ∇⊥, (2.42)

and can think of the vector derivative as the projection of the gradient onto the tangent space at the point of evaluation. Please see [18] for an excellent introduction of the reciprocal frame, the gradient, and the vector derivative, and for details about the connectivity of the manifold ignored here.

2.2.5 Examples.

We’ve just blasted through a few abstract ideas:

• The curvilinear representation of the gradient.

• The gradient representation of the reciprocal frame.

• The vector derivative.

This completes the mathematical preliminaries required to formulate geometric calculus, the multivector generalization of line, surface, and volume integrals. Before diving into the calculus let’s consider some example parameterizations to illustrate how some of the new ideas above ﬁt together.

2.2.5.1 Example parameterization: Polar coordinates.

We will now consider a simple concrete example of a vector parameterization, that of polar coordinates in R2

x(ρ, φ) = ρe1 exp (e12φ) , (2.43)

as illustrated in ﬁg. 2.5. Using this example we will 2.2 curvilinear coordinates. 81

3.0

2.5

2.0

x ρρ 1.5

e2 1.0

ρ 0.5

θ e1 0.5 1.0 1.5 2.0 2.5 3.0 Figure 2.5: Polar coordinates.

• Compute the curvilinear coordinates. We will refer to these as xρ, xφ, instead of x1, x2.

• Find the squared length of xρ, xφ, and show that they are perpendicular (but not orthonormal.)

• Perform a ﬁrst bivector valued integral.

• Compute the reciprocal frame vectors with geometric arguments.

• Compute the reciprocal frame explicitly from the gradients of the coordinates.

• Find the polar form of the gradient with respect to this parameterization.

Curvilinear coordinates. The curvilinear coordinate basis can be computed directly

∂ x = ρe exp (e φ) ρ ∂ρ 1 12 (2.44a) = e1 exp (e12φ)

∂ xφ = ρe1 exp (e12φ) ∂φ (2.44b) = ρe1e12 exp (e12φ) = ρe2 exp (e12φ) . 82 multivector calculus.

Normality. To show that these vectors are perpendicular, we can select the scalar grade of their product, and use theorem 1.11, property (c) to swap the vector and complex exponential, conjugating the exponential

xρ · xφ = e1 exp (e12φ) ρe2 exp (e12φ)

= ρ e1 exp (e12φ) exp (−e12φ) e2 (2.45) = ρhe1e2i = 0.

Length of basis elements. We can use the same method to ﬁnd the (squared) length of the vectors

2 xρ = e1 exp (e12φ) e1 exp (e12φ) − = e1 exp (e12φ) exp ( e12φ) e1 (2.46) D 2E = e1 = 1,

and

2 xφ = ρe2 exp (e12φ) ρe2 exp (e12φ) = ρ2 e exp (e φ) exp (−e φ) e 2 12 12 2 (2.47) 2D 2E = ρ e2 = ρ2.

A bivector integral. One of our goals is to understand the multivector generalization of Stokes’ theorem and the divergence theorem, but even before that, we can evaluate some simple multivector integrals. In particular, we can calculate the (oriented) area of a circle, given a bivector representation of the area element. 2.2 curvilinear coordinates. 83

Z r Z 2π Z r Z 2π dxρ ∧ dxφ = dρdφ xρ ∧ xφ ρ =0 φ =0 ρ=0 φ=0 Z r Z 2π D E = dρdφ x x ρ φ 2 ρ=0 φ=0 Z r Z 2π

= dρdφ e1 exp (e12φ) ρe2 exp (e12φ) 2 ρ=0 φ=0 (2.48) Z r Z 2π

= ρdρdφ e1e2 exp (−e12φ) exp (e12φ) 2 ρ=0 φ=0 Z r Z 2π = ρdρdφ e12 ρ=0 φ=0 2 = πr e12.

Integrating the bivector area over a circular region gives us the area of that region, but weighted by the R2 pseudoscalar. This is an oriented area.

Reciprocal basis. Because xρ, xφ are mutually perpendicular, we have only to rescale them to determine the reciprocal basis, and can do so by inspection

ρ x = e1 exp (e12φ) 1 (2.49) xφ = e exp (e φ) . ρ 2 12 According to theorem 2.1 we should be able to ﬁnd eq. (2.49) by computing the gradients of ρ and φ respectively. If we do so using the R2 standard basis representation of the gradient, we must ﬁrst solve for ρ = ρ(x, y), φ = φ(x, y), inverting

x = ρ cos φ (2.50) y = ρ sin φ.

An implicit solution to this inversion problem is

ρ2 = x2 + y2 (2.51) tan φ = y/x, 84 multivector calculus.

which we can implicitly diﬀerentiate to evaluate the components of the desired gradients ∂ρ 2ρ = 2x ∂x ∂ρ 2ρ = 2y ∂y 1 ∂φ y (2.52) = − cos2 φ ∂x x2 1 ∂φ 1 = . cos2 φ ∂y x The gradients are therefore

1 ∇ρ = (cos φ, sin φ) ρ (2.53a) e12φ = e1e = xρ

! y 1 ∇φ = cos2 φ − , x2 x 1 = (− sin φ, cos φ) ρ e (2.53b) = 2 (cos φ + e sin φ) ρ 12 e2 = ee12φ ρ = xφ,

which is consistent with eq. (2.49), as expected.

Gradient. The polar form of the R2 gradient is

∂ ∂ ∇ = xρ + xφ ∂ρ ∂φ (2.54) ∂ 1 ∂ = ρˆ + φˆ , ∂ρ ρ ∂φ where ρ ρˆ = xρ = e1 exp (e12φ) = x 1 (2.55) φˆ = x = e exp (e φ) = ρxφ. ρ φ 2 12 2.2 curvilinear coordinates. 85

Should we extend this vector space to R3, the parameterization of eq. (2.43) covers the subspace of the x-y plane, and for that subspace, the vector derivative is

∂ ∂ ∂ = xρ + xφ ∂ρ ∂φ (2.56) ∂ 1 ∂ = ρˆ + φˆ . ∂ρ ρ ∂φ

2.2.5.2 Example parameterization: Spherical coordinates.

The spherical vector parameterization admits a compact GA representation. From the coordinate representation, some factoring gives

x = r (e1 sin θ cos φ + e2 sin θ sin φ + e3 cos θ) = r (sin θe1(cos φ + e12 sin φ) + e3 cos θ) e12φ (2.57) = r sin θe1e + e3 cos θ e12φ = re3 cos θ + sin θe3e1e .

With

i = e12 iφ (2.58) j = e31e , this is jθ x = re3e . (2.59)

The curvilinear basis can be easily be computed in software

In[13]:= ClearAll[i,j, ej,x, xr, xt, xp] i=e[1, 2]; j[phi_] = GeometricProduct[e[3, 1], Cos[phi] +i Sin[phi]]; ej[t_, p_] = Cos[t] +j[p] Sin[t]; x[r_, t_, p_] =r GeometricProduct[e[3], ej[t,p]];

xr[r_, theta_, phi_] =D[x[a, theta, phi],a] /.a →r; xt[r_, theta_, phi_] =D[x[r,t, phi],t] /.t →theta; xp[r_, theta_, phi_] =D[x[r, theta,p],p] /.p →phi;

{x[r, θ, φ], xr[r, θ, φ], xt[r, θ, φ], xp[r, θ, φ]} // Column 86 multivector calculus.

Out[13]= r (Cos[θ] e[3] + Cos[φ] e[1] Sin[θ] + e[2] Sin[θ] Sin[φ]) Cos[θ] e[3] + Cos[φ] e[1] Sin[θ] + e[2] Sin[ θ] Sin[φ] r (Cos[θ] Cos[φ] e[1] - e[3] Sin[θ] + Cos[θ] e[2] Sin[φ]) r (Cos[φ] e[2] Sin[θ] - e[1] Sin[θ] Sin[φ])

Unfortunately the compact representation is lost doing so. Computing the basis elements manually, we ﬁnd jθ xr = e3e (2.60a)

jθ xθ = re3 je iφ jθ (2.60b) = re3e31e e iφ jθ = re1e e

∂ iφ xφ = re3 sin θe31e ∂φ (2.60c) iφ = r sin θe1e12e iφ = r sin θe2e . These are all mutually normal, which can be veriﬁed by computing dot products.

In[14]:= ClearAll[x1, x2, x3] x1= xr[r, θ, φ]; x2= xt[r, θ, φ]; x3= xp[r, θ, φ]; MapThread[InnerProduct, {{x1, x2, x3}, {x2, x3, x1}}]// Simplify

Out[14]= {0,0,0}

An algebraic computation of these dot products is left as a problem for the student (exercise 2.4). Orthonormalization of the curvilinear basis is now possible by inspection jθ rˆ = xr = e3e 1 θˆ = x = e eiφe jθ r θ 1 (2.61) 1 φˆ = x = e eiφ, r sin θ φ 2 so r jθ x = rˆ = e3e 1 1 xθ = θˆ = e eiφe jθ r r 1 (2.62) 1 1 xφ = φˆ = e eiφ. r sin θ r sin θ 2 2.2 curvilinear coordinates. 87

In particular, this shows that the spherical representation of the gradient is ∂ ∂ ∂ ∇ = xr + xθ + xφ ∂r ∂θ ∂φ (2.63) ∂ 1 ∂ 1 ∂ = rˆ + θˆ + φˆ . ∂r r ∂θ r sin θ ∂φ The spherical (oriented) volume element can also be computed in a compact fashion

d3x = x ∧ x ∧ x drdθdφ r θ φ D E = x x x r θ φ 3 D jθ iφ jθ iφE (2.64) = e3e re1e e r sin θe2e D E3 = r2 sin θ e e jθe eiφe jθe eiφ 3 1 2 3 2 = r sin θ e123. The scalar factor is in fact the Jacobian with respect to the spherical parameterization dV ∂(x , x , x ) = 1 2 3 drdθdφ ∂(r, θ, φ)

sin θ cos φ sin θ sin φ cos θ (2.65) = r cos θ cos φ r cos θ sin φ −r sin θ

−r sin θ sin φ r sin θ cos φ 0 = r2 sin θ. The ﬁnal reduction of eq. (2.64), and the expansion of the Jacobian eq. (2.65), are both easily veriﬁed with software

In[15]:= OuterProduct[ xr[r, θ, φ], xt[r, θ, φ], xp[r, θ, φ]]

{e1,e2,e3} = IdentityMatrix[3]; jacobian={xr[r, θ, φ], xt[r, θ, φ], xp[r, θ, φ]} /. {e[1] → e1,e[2] → e2,e[3] →e3}; Det[ jacobian]// Simplify 2 Out[15]= r e[1,2,3] Sin[θ] 2 Out[16]= r Sin[θ] Performing these calculations manually are left as problems for the student (exercise 2.6, exercise 2.5). 88 multivector calculus.

2.2.5.3 Example parameterization: Toroidal coordinates.

Figure 2.6: Toroidal parameterization.

Here is a 3D example of a parameterization with a non-normal curvilinear basis, that of a toroidal subspace speciﬁed by two angles and a radial distance to the center of the toroid, as illustrated in ﬁg. 2.6. The position vector on the surface of a toroid of radius ρ within the torus can be stated directly

− jθ/2 iφ jθ/2 x(ρ, θ, φ) = e ρe1e + Re3 e (2.66a)

i = e1e3 (2.66b)

j = e3e2 (2.66c)

It happens that the unit bivectors i and j used in this construction happen to have the quaternion- ic properties i j = − ji, and i2 = j2 = −1 which can be veriﬁed easily. After some regrouping the curvilinear basis is found to be

∂x x = = e− jθ/2e eiφe jθ/2 (2.67a) ρ ∂ρ 1 ∂x x = = e− jθ/2 (R + ρ sin φ) e e jθ/2 (2.67b) θ ∂θ 2 ∂x x = = e− jθ/2ρe eiφe jθ/2. (2.67c) φ ∂φ 3 2.2 curvilinear coordinates. 89

The oriented volume element can be computed using a trivector selection operation, which conveniently wipes out a number of the interior exponentials ∂x ∂x ∂x D E ∧ ∧ = ρ (R + ρ sin φ) e− jθ/2e eiφe e eiφe jθ/2 . (2.68) ∂ρ ∂θ ∂φ 1 2 3 3

− jθ/2 Note that e1 commutes with j = e3e2, so also with e . Also e2e3 = − j anticommutes with i, so there is a conjugate commutation eﬀect eiφ j = je−iφ. This gives D E D E e− jθ/2e eiφe e eiφe jθ/2 = − e e− jθ/2 je−iφeiφe jθ/2 1 2 3 3 1 3 D E = − e e− jθ/2 je jθ/2 1 3 (2.69) = −he1 ji3 = I.

Together the trivector grade selection reduces almost magically to just

∂x ∂x ∂x ∧ ∧ = ρ (R + ρ sin φ) I. (2.70) ∂ρ ∂θ ∂φ

FIXME: show this with Mathematica too. Thus the (scalar) volume element is

dV = ρ (R + ρ sin φ) dρdθdφ. (2.71)

As a check, it should be the case that the volume of the complete torus using this volume element has the expected V = (2πR)(πr2) value. That volume is

Z r Z 2π Z 2π V = ρ (R + ρ sin φ) dρdθdφ. (2.72) ρ=0 θ=0 φ=0

The sine term conveniently vanishes over the 2π interval, leaving just

1 V = r2R(2π)(2π), (2.73) 2 as expected.

2.2.6 Problems.

Exercise 2.4 Spherical coordinate basis normality. 90 multivector calculus.

Using scalar selection, show that the spherical curvilinear basis of eq. (2.60) are all mutually normal. Exercise 2.5 Spherical volume element pseudoscalar. Using geometric algebra, perform the reduction of the grade three selection made in the ﬁnal step of eq. (2.64).

Exercise 2.6 Spherical volume Jacobian. Without software, expand and simplify the determinant of eq. (2.65).

2.3 integration theory.

2.3.1 Hypervolume integral

We wish to generalize the concepts of line, surface and volume integrals to hypervolumes and multivector functions, and deﬁne a hypervolume integral as

Deﬁnition 2.4: Multivector integral.

Given a hypervolume parameterized by k parameters, k-volume volume element dkx, and multivector functions F, G, a k-volume integral with the vector derivative acting to the right on G is written as

Z → dkx∂G, V a k-volume integral with the vector derivative acting to the left on F is written as

Z ← Fdkx∂, V and a k-volume integral with the vector derivative acting bidirectionally on F, G is written as

Z ↔ Z ← Z → Fdkx∂G ≡ Fdkx∂ G + Fdkx ∂G . V V V 2.3 integration theory. 91

The explicit meaning of these directional acting derivative operations is given by the chain rule coordinate expansion   ↔ X ↔ k k  i  Fd x ∂ G = Fd x  x ∂i G i k X i k X i = (∂iF)d x x G + Fd x x (∂iG) i i ← → ≡ (Fdkx∂)G + Fdkx(∂G),

with ∂ acting on F and G, but not the volume element dkx, which may also be a function of the implied parameterization.

The vector derivative may not commute with F, G nor the volume element dkx, so we are forced to use some notation to indicate what the vector derivative (or gradient) acts on. In conventional right acting cases, where there is no ambiguity, arrows will usually be omitted, but braces may also be used to indicate the scope of derivative operators. This bidirectional notation will also be used for the gradient, especially for volume integrals in R3 where the vector derivative is identical to the gradient. Some authors use the Hestenes dot notation, with overdots or primes to indicating the exact scope of multivector derivative operators, as in

Fd˙ kx∂˙G˙ = Fd˙ kx∂˙G + Fdkx∂˙G˙. (2.77)

The dot notation has the advantage of emphasizing that the action of the vector derivative (or gradient) is on the functions F, G, and not on the hypervolume element dkx. However, in this book, where primed operators such as ∇0 are used to indicate that derivatives are taken with respect to primed x0 variables, a mix of dots and ticks would have been confusing.

2.3.2 Fundamental theorem.

The fundamental theorem of geometric calculus is a generalization of many conventional scalar and vector integral theorems, and relates a hypervolume integral to its boundary. This is a a powerful theorem, which we will use with Green’s functions to solve Maxwell’s equation, but also to derive the geometric algebra form of Stokes’ theorem, from which most of the familiar integral calculus results follow.

Theorem 2.3: Fundamental theorem of geometric calculus 92 multivector calculus.

Given multivectors F, G, a parameterization x = x(u1, u2, ···), with hypervolume element k k d x = d uIk, where Ik = x1 ∧ x2 ∧ · · · ∧ xk, the hypervolume integral is related to the boundary integral by

Z ↔ Z Fdkx∂G = Fdk−1xG, V ∂V

where ∂V represents the boundary of the volume, and dk−1x is the hypersurface element. This is called the Fundamental theorem of geometric calculus. The hypersurface element and boundary integral is deﬁned for k > 1 as Z Z k−1 X k−1 i Fd xG ≡ d ui F Ik · x G , ∆ui ∂V i

k−1 where d ui is the product of all du j except for dui. For k = 1 the hypersurface element and associated boundary “integral” is really just convenient general shorthand, and should be taken to mean the evaluation of the FG multivector product over the range of the parameter Z 0 ≡ | Fd xG FG ∆u1 . ∂V

The geometry of the hypersurface element dk−1x will be made more clear when we consider the speciﬁc cases of k = 1, 2, 3, representing generalized line, surface, and volume integrals respectively. Instead of terrorizing the reader with a general proof theorem 2.3, which requires some unpleasant index gymnastics, this book will separately state and prove the fundamental theorem of calculus for each of the k = 1, 2, 3 cases that are of interest for problems in R2 and R3. For the interested reader, a sketch of the general proof of theorem 2.3 is available in appendixB. Before moving on to the line, surface, and volume integral cases, we will state and prove the general Stokes’ theorem in its geometric algebra form.

2.3.3 Stokes’ theorem.

An important consequence of the fundamental theorem of geometric calculus is the geometric algebra generalization of Stokes’ theorem. The Stokes’ theorem that we know from conventional vector calculus relates R3 surface integrals to the line integral around a bounding surface. The geometric algebra form of Stokes’ theorem is equivalent to Stokes’ theorem from the theory of diﬀerential forms, which relates hypervolume integrals of blades5 to the integrals over their hypersurface boundaries, a much more general result.

5 Blades are isomorphic to the k-forms found in the theory of diﬀerential forms. 2.3 integration theory. 93

Theorem 2.4: Stokes’ theorem

Stokes’ theorem relates the dot product of a k volume element dkx with the wedge product “curl” of an s-blade F, s < k as follows Z Z dkx · (∂ ∧ F) = dk−1x · F. V ∂V

We will see that most of the well known scalar and vector integral theorems can easily be derived as direct consequences of theorem 2.4, itself a special case of theorem 2.3. We can prove Stokes’ theorem from theorem 2.3 by setting F = 1, and requiring that G is an s-blade, with grade s < k. The proof follows by selecting the k − (s + 1) grade, the lowest grade of dkx(∂ ∧ G), from both sides of theorem 2.3. For the grade selection of the hypervolume integral we have *Z + *Z Z + dkx∂G = dkx(∂ · G) + dkx(∂ ∧ G) , (2.78) V k−(s+1) V V k−(s−1) however, the lowest grade of dkx(∂ · G) is k − (s − 1) = k − s + 1 > k − (s + 1), so the divergence integral is zero. As dk−1x is a k − 1 blade

Z Z D E dkx · (∂ ∧ G) = dk−1xG k−(s+1) V Z∂V (2.79) = dk−1x · G, ∂V proving the theorem.

2.3.4 Line integral.

A single parameter curve, and the corresponding differential with respect to that parameter, is plotted in fig. 2.7. The differential with respect to the parameter a is

∂x dx = da = x da. (2.80) a ∂a a 94 multivector calculus.

Figure 2.7: One parameter manifold.

The vector derivative has just one component

X i ∂ = x (xi · ∇) i ∂ (2.81) = xa ∂a a ≡ x ∂a.

The line integral specialization of deﬁnition 2.4 can now be stated

Deﬁnition 2.5: Multivector line integral.

Given an connected curve C parameterized by a single parameter, and multivector functions F, G, we deﬁne the line integral as

Z ↔ Z ← Z → Fd1x∂G ≡ Fd1x∂ G + Fd1x ∂G , C C C

1 where the one parameter diﬀerential form d x = da xa varies over the curve.

The line integral specialization of theorem 2.3 is

Theorem 2.5: Multivector line integral.

Given a connected curve C parameterized by a single parameter, and multivector functions F, G, the line integral is related to the boundary by Z Fdx∂G = FG|∆a. C 2.3 integration theory. 95

The proof follows by expansion. For the (single variable) parameterization a above

Z ↔ Z ← Z → Fd1x ∂ G = Fd1x∂ G + Fd1x ∂G C ZC ZC ∂F a a ∂G = daxax G + Fdaxax C ∂a C ∂a Z ∂F Z ∂G (2.82) = da G + daF C ∂a C ∂a Z ∂ = da (FG) C ∂a = F(a1)G(a1) − F(a0)G(a0), where the boundaries of the parameterization have been assumed to be C : a ∈ [a0, a1]. We a have a perfect cancellation of the reciprocal frame x with the vector xa that lies along the a curve, since x xa = 1. This leaves a perfect derivative of the product of FG, which can be integrated over the length of the curve, yielding the diﬀerence of the product with respect to the parameterization of the end points of the curve. For a single parameter subspace the reciprocal frame vector xa is trivial to calculate, as it is a 2 just the inverse of xa, that is x = xa/kxak . Observe that we did not actually have to calculate it, but instead only require that the vector is invertible. An important (and familiar) special case of theorem 2.5 is the fundamental theorem of calculus for line integrals, which can be obtained by using a single scalar function f

Theorem 2.6: Line integral of a scalar function (Stokes’).

Given a scalar function f , its line integral is given by Z Z dx · ∂ f = dx · ∇ f = f |∆a. C C

Writing out theorem 2.5 with F = 1, G = f (x(a)), we have Z 1 d x∂ f = f |∆a. (2.83) C This is a multivector equation with scalar and bivector grades on the left hand side, but only scalar grades on the right. Equating grades yields two equations Z 1 d x · ∂ f = f |∆a (2.84a) C Z d1x ∧ ∂ f = 0 (2.84b) C 96 multivector calculus.

Because d1x · ∂ = d1x · ∇, we can replace the vector derivative with the gradient in eq. (2.84a), which yields the conventional line integral result, proving the theorem.

2.3.5 Surface integral.

A two parameter curve, and the corresponding diﬀerentials with respect to those parameters, is plotted in ﬁg. 2.8.

Figure 2.8: Two parameter manifold diﬀerentials.

Given parameters a, b, the diﬀerentials along each of the parameterization directions are ∂x dxa = da = xada ∂a (2.85) ∂x dx = db = x db. b ∂b b The bivector valued surface area element for this parameterization is

2 d x = dxa ∧ dxb = dadb(xa ∧ xb). (2.86) 2.3 integration theory. 97

The vector derivative, the projection of the gradient onto the surface at the point of integration (also called the tangent space), now has two components

X i ∂ = x (xi · ∇) i ∂ ∂ (2.87) = xa + xb ∂a ∂b a b ≡ x ∂a + x ∂b.

The surface integral specialization of deﬁnition 2.4 can now be stated

Deﬁnition 2.6: Multivector surface integral.

Given an connected surface S parameterized by two parameters, and multivector functions F, G, we deﬁne the surface integral as

Z Z ← Z → Fd2x∂G ≡ Fd2x∂ G + Fd2x ∂G , S S S

2 where the two parameter diﬀerential form d x = dadb xa ∧ xb varies over the surface.

The surface integral specialization of theorem 2.3 is

Theorem 2.7: Multivector surface integral.

x Given a connected surface S with an area element d x = dx1 ∧ dx2, and multivector functions F, G, the surface integral is related to the boundary by

Z ↔ Fd2x∂G = FdxG, S ∂S where ∂S is the boundary of the surface S .

2 2 In R with d x = idA, i = e12, this may be written Z Fi∇G dA = FdxG. (2.88) S ∂S

As i does not commute with all R2 multivectors, unless F = 1 we cannot generally pull i out of the integral. In R3, with d2x = InˆdA, we may use a scalar area element, but cannot generally replace the vector derivative with the gradient. 98 multivector calculus.

To see why this works, we would ﬁrst like to reduce the product of the area element and the vector derivative 2 a b d x∂ = dadb (xa ∧ xb) x ∂a + x ∂b . (2.89)

a Since x ∈ span {xa, xb}, this multivector product has only a vector grade. That is

a a ((((a (xa ∧ xb) x = (xa ∧ xb) · x + ((x(a ∧(xb) ∧ x a = (xa ∧ xb) · x (2.90) a a = xa xb · x − xb xa · x = −xb.

Similarly

 b b b (xa ∧ xb) x = (xa ∧ xb) · x + (xa ∧ xb) ∧ x b = (xa ∧ xb) · x (2.91) b b = xa xb · x − xb xa · x = xa,

so 2 d x∂ = xa∂b − xb∂a. (2.92)

Inserting this into the surface integral, we ﬁnd Z Z ← Z → Fd2x∂G = Fd2x∂ G + Fd2x ∂G S ZS S Z = dadb (∂bFxa − ∂aFxb) G + dadb F (xa∂bG − xb∂aG) S ! S ! Z ∂F ∂x ∂F ∂x Z ∂x ∂G ∂x ∂G = dadb − G + dadb F − S ∂b ∂a ∂a ∂b S ∂a ∂b ∂b ∂a ! ! ! Z ∂ ∂x Z ∂ ∂x Z ∂ ∂x ∂ ∂x = dadb F G − dadb F G − dadb F − G S ∂b ∂a S ∂a ∂b S ∂b ∂a ∂a ∂b ! ! Z ∂ ∂x Z ∂ ∂x = dadb F G − dadb F G . S ∂b ∂a S ∂a ∂b (2.93)

This leaves two perfect diﬀerentials, which can both be integrated separately. That gives

Z Z ! Z ! 2 ∂x ∂x Fd x∂G = da F G − db F G S ∆a ∂a ∆b ∂b Z ∆bZ ∆a (2.94) = (FdxaG)|∆b − (FdxbG)|∆a. ∆a ∆b 2.3 integration theory. 99

Figure 2.9: Contour for two parameter surface boundary.

Suppose we are integrating over the unit parameter volume space [a, b] ∈ [0, 1] ⊗ [0, 1] as illustrated in fig. 2.9. Comparing to the figure we see that we’ve ended up with a clockwise line integral around the boundary of the surface. For a given subset of the surface, the bivector area element can be chosen small enough that it lies in the tangent space to the surface at the point of integration. In that case, a larger bounding loop can be conceptualized as the sum of a number of smaller ones, as sketched in fig. 2.10, in which case the contributions of the interior loop segments cancel out.

2.3.6 Two parameter Stokes’ theorem.

Two special cases of theorem 2.7 when scalar and vector functions are integrated over a surface. For scalar functions we have

Theorem 2.8: Surface integral of scalar function (Stokes’).

Given a scalar function f (x) its surface integral is given by Z Z d2x · ∂ f = d2x · ∇ f = dx f. S S ∂S

100 multivector calculus.

Figure 2.10: Sum of inﬁnitesimal loops.

In R3, this can be written as Z dA nˆ × ∇ f = dx f, S ∂S

where nˆ is the normal speciﬁed by d2x = InˆdA.

To show the ﬁrst part, we can split the (multivector) surface integral into vector and trivector grades Z Z Z d2x∂ f = d2x · ∂ f + d2x ∧ ∂ f. (2.95) S S S a b 2 Since x , x both lie in the span of {xa, xb}, d x ∧ ∂ = 0, killing the second integral in eq. (2.95). If the gradient is decomposed into its projection along the tangent space (the vector derivative) and its perpendicular components, only the vector derivative components of the gradient contribute to its dot product with the area element. That is

2 2 a b d x · ∇ = d x · x ∂a + x ∂b + ··· 2 a b (2.96) = d x · x ∂a + x ∂b = d2x · ∂.

This means that for a scalar function Z Z d2x∂ f = d2x · ∇ f. (2.97) S S 2.3 integration theory. 101

The second part of the theorem follows by grade selection, and application of a duality transformation for the area element

D E d2x · ∇ f = d2x∇ f 1 = dAhInˆ∇ f i1 (2.98) = dAhI (nˆ · ∇ f + Inˆ × ∇ f )i1 = −dAnˆ × ∇ f.

back substitution of eq. (2.98) completes the proof of theorem 2.8. For vector functions we have

Theorem 2.9: Surface integral of a vector function (Stokes’).

Given a vector function f(x), the surface integral is given by Z d2x · (∇ ∧ f) = dx · f. S ∂S

In R3, this can be written as Z dA nˆ · (∇ × f) = dx · f, S ∂S

where nˆ is the normal speciﬁed by d2x = InˆdA.

2.3.7 Green’s theorem.

Theorem 2.9, when stated in terms of coordinates, is another well known result.

Theorem 2.10: Green’s theorem.

P i N Given a vector f = i fix in R , and a surface parameterized by x = x(u1, u2), Green’s theorem states Z ! ∂ f1 ∂ f2 du1du2 − = du1 f1 + du2 f2. S ∂u2 ∂u1 ∂S

102 multivector calculus.

2 This is often stated for vectors f = Pe1 + Qe2 ∈ R with a Cartesian x, y parameterization as ! Z ∂P ∂Q dxdy − = Pdx + Qdy. S ∂y ∂x ∂S

FIXME: Add an example (lots to pick from in any 3rd term calc text) The ﬁrst equality in theorem 2.10 holds in RN for vectors expressed in terms of an arbitrary curvilinear basis. Only the (curvilinear) coordinates of the vector f contribute to this integral, and only those that lie in the tangent space. The reciprocal basis vectors xi are also nowhere to be seen. This is because they are either obliterated in dot products with x j, or cancel due to mixed partial equality. To see how this occurs let’s look at the area integrand of theorem 2.9   X  d2x · (∇ ∧ f) = du du (x ∧ x ) ·  xi∂ ∧ f x j  1 2 1 2  i j  i j X i j = du1du2 (x1 ∧ x2) · x · ∂i( f jx ) i j X i j X i j = du1du2 (x1 ∧ x2) · x · x ∂i f j + du1du2 f j (x1 ∧ x2) · x · (∂ix ). i j i j (2.99)

With a bit of trouble, we will see that the second integrand is zero. On the other hand, the ﬁrst integrand simpliﬁes without too much trouble

X i j X j (x1 ∧ x2) · x · x ∂i f j = (x1δ2i − x2δ1i) · x ∂i f j i j i j X j j (2.100) = x1 · x ∂2 f j − x2 · x ∂1 f j j = ∂2 f1 − ∂1 f2.

For the second integrand, we have

X i j X X f j (x1 ∧ x2) · x · (∂ix ) = f j (x1δ2i − x2δ1i) · (∂ix j) i j j i (2.101) X j j = f j x1 · (∂2x ) − x2 · (∂1x ) j 2.3 integration theory. 103

We can apply the chain rule (backwards) to the portion in brackets to ﬁnd j j j j j j x1 · (∂2x ) − x2 · (∂1x ) = ∂2x1 · x − (∂2x1) · x − ∂1x2 · x + (∂1x2) · x = x j · (∂1x2 − ∂2x1) ! ∂ ∂x ∂ ∂x (2.102) = x j · − ∂u1 ∂u2 ∂u2 ∂u1 = 0.

j In this reduction the derivatives of xi · x = δi j were killed since those are constants (either zero or one). The ﬁnal step relies on the fact that we assume our vector parameterization is well behaved enough that the mixed partials are zero. Substituting these results into theorem 2.9 we ﬁnd

  X  · ·  i dx f = (du1x1 + du2x2)  fix  ∂S ∂S i (2.103) = du1 f1 + du2 f2 Z∂S

= du1du2 (∂2 f1 − ∂1 f2) , S which completes the proof.

2.3.8 Volume integral.

A three parameter curve, and the corresponding differentials with respect to those parameters, is sketched in fig. 2.11. Given parameters u1, u2, u3, we can denote the differentials along each of the parameterization directions as ∂x dx1 = du1 = x1du1 ∂u1 ∂x dx2 = du2 = x2du2 (2.104) ∂u2 ∂x dx3 = du3 = x3du3. ∂u3 The trivector valued volume element for this parameterization is

3 3 d x = dx1 ∧ dx1 ∧ dx1 = d u (x1 ∧ x2 ∧ x3), (2.105) 104 multivector calculus.

Figure 2.11: Three parameter volume element.

3 where d u = du1du2du3. The vector derivative, the projection of the gradient onto the volume at the point of integration (also called the tangent space), now has three components

X i ∂ = x (xi · ∇) i ∂ ∂ ∂ (2.106) = x1 + x2 + x3 ∂u1 ∂u2 ∂u3 1 2 3 ≡ x ∂1 + x ∂2 + x ∂3.

The volume integral specialization of deﬁnition 2.4 can now be stated

Deﬁnition 2.7: Multivector volume integral.

Given an connected volume V parameterized by two parameters, and multivector functions F, G, we deﬁne the volume integral as

Z ↔ Z ← Z → Fd3x∂G ≡ Fd3x∂ G + Fd3x ∂G , V V V

3 3 3 where the three parameter diﬀerential form d x = d u x1 ∧ x2 ∧ x3, d u = du1du2du3 varies ↔ over the volume, and ∂ acts on F, G, but not the volume element d2x. 2.3 integration theory. 105

The volume integral specialization of theorem 2.3 is

Theorem 2.11: Multivector volume integral.

3 Given a connected volume V with a volume element d x = dx1 ∧ dx2 ∧ dx3, and multivector functions F, G, a volume integral can be reduced to a surface integral as follows

Z ↔ Fd3x∂G = Fd2xG, V ∂V

where ∂V is the boundary of the volume V, and d2x is the counterclockwise oriented area element on the boundary of the volume. In R3 with d3x = IdV, d2x = InˆdA, this integral can be written using a scalar volume element

Z ↔ Z dV F ∂G = dA FnˆG. V ∂V

To see why this works, and deﬁne d2x more precisely, we would ﬁrst like to reduce the product of the volume element and the vector derivative

3 3 1 2 3 d x∂ = d u (x1 ∧ x2 ∧ x3) x ∂1 + x ∂2 + x ∂3 . (2.107)

i Since all x lie within span {x1, x2, x3}, this multivector product has only a vector grade. That is (( i i (((( i (x1 ∧ x2 ∧ x3) x = (x1 ∧ x2 ∧ x3) · x + ((x(1 ∧(x2 ∧ x3) ∧ x , (2.108) for all xi. These products reduces to

1 (x2 ∧ x3 ∧ x1) x = x2 ∧ x3 2 (x3 ∧ x1 ∧ x2) x = x3 ∧ x1 (2.109) 3 (x1 ∧ x2 ∧ x3) x = x1 ∧ x2. 106 multivector calculus.

Inserting eq. (2.109) into the volume integral, we ﬁnd

Z Z ← Z → Fd3x∂G = Fd3x∂ G + Fd3x ∂G V ZV V 3 = d u ((∂1F)x2 ∧ x3G + (∂2F)x3 ∧ x1G + (∂3F)x1 ∧ x2G) VZ 3 + d u (Fx2 ∧ x3(∂1G) + Fx3 ∧ x1(∂2G) + Fx1 ∧ x2(∂3G)) Z V 3 = d u (∂1(Fx2 ∧ x3G) + ∂2(Fx3 ∧ x1G) + ∂3(Fx1 ∧ x2G)) (2.110) VZ 3 − d u (F(∂1(x2 ∧ x3))G + F(∂2(x3 ∧ x1))G + F(∂3(x1 ∧ x2))G) Z V 3 = d u (∂1(Fx2 ∧ x3G) + ∂2(Fx3 ∧ x1G) + ∂3(Fx1 ∧ x2G)) VZ 3 − d u F (∂1(x2 ∧ x3) + ∂2(x3 ∧ x1) + ∂3(x1 ∧ x2)) G. V The sum within the second integral is

3 X i 3 1 2 ∂i Ik · x = ∂3 (x1 ∧ x2 ∧ x3) · x + ∂1 (x2 ∧ x3 ∧ x1) · x + ∂2 (x3 ∧ x1 ∧ x2) · x i=1

= ∂3 (x1 ∧ x2) + ∂1 (x2 ∧ x3) + ∂2 (x3 ∧ x1)

= (∂3x1) ∧ x2 + x1 ∧ (∂3x2)

+ (∂1x2) ∧ x3 + x2 ∧ (∂1x3)

+ (∂2x3) ∧ x1 + x3 ∧ (∂2x1)

= x2 ∧ (−∂3x1 + ∂1x3) + x3 ∧ (−∂1x2 + ∂2x1) + x1 ∧ (−∂2x3 + ∂3x2) ! ! ! ∂2x ∂2x ∂2x ∂2x ∂2x ∂2x = x2 ∧ − + + x3 ∧ − + + x1 ∧ − + , ∂3∂1 ∂1∂3 ∂1∂2 ∂2∂1 ∂2∂3 ∂3∂2 (2.111)

which is zero by equality of mixed partials. This leaves three perfect diﬀerentials, which can integrated separately, giving Z Z Z 3 ∧ | ∧ | Fd x∂G = du2du3 (Fx2 x3G) ∆u1 + du3du1 (Fx3 x1G) ∆u2 V Z ∧ | + du1du2 (Fx1 x2G) ∆u3 Z Z Z ∧ | ∧ | ∧ | = (Fdx2 dx3G) ∆u1 + (Fdx3 dx1G) ∆u2 + (Fdx1 dx2G) ∆u3 . (2.112) 2.3 integration theory. 107

This proves the theorem from an algebraic point of view. With the aid of a geometrical model, such as that of ﬁg. 2.12, if assuming that dx1, dx2, dx3 is a right handed triple). it is possible to convince oneself that the two parameter integrands describe an integral over a counterclockwise oriented surface (

(a) (b)

Figure 2.12: Diﬀerential surface of a volume.

We obtain the RHS of theorem 2.11 if we introduce a mnemonic for the bounding oriented surface of the volume 2 d x ≡ dx1 ∧ dx2 + dx2 ∧ dx3 + dx3 ∧ dx1, (2.113) where it is implied that each component of this area element and anything that it is multiplied with is evaluated on the boundaries of the integration volume (for the parameter omitted) as detailed explicitly in eq. (2.112).

2.3.9 Three parameter Stokes’ theorem.

Three special cases of theorem 2.11 can be obtained by integrating scalar, vector or bivector functions over the volume, as follows 108 multivector calculus.

Theorem 2.12: Volume integral of scalar function (Stokes’).

Given a scalar function f (x) its volume integral is given by Z Z d3x · ∂ f = d3x · ∇ f = d2x f. V V ∂V

2.3 integration theory. 109

In R3, this can be written as Z Z dV∇ f = dAnˆ f V ∂V where nˆ is the outwards normal speciﬁed by d2x = InˆdA, and d3x = IdV.

Theorem 2.13: Volume integral of vector function (Stokes’).

The specialization of Stokes’ theorem for a volume integral of the (bivector) curl of a vector function f(x), relates the volume integral to a surface area over the boundary as follows Z Z d3x · (∂ ∧ f) = d3x · (∇ ∧ f) = d2x · f. V V ∂V

In R3, this can be written as Z Z dV ∇ × f = dA nˆ × f, V ∂V or with a duality transformation f = IB, where B is a bivector Z Z dV ∇ · B = dA nˆ · B, V ∂V where nˆ is the normal speciﬁed by d2x = InˆdA, and d3x = IdV.

Theorem 2.14: Volume integral of bivector function (Stokes’, divergence).

Given a bivector function B(x), the volume integral of the (trivector) curl is related to a surface integral by Z Z d3x · (∂ ∧ B) = d3x · (∇ ∧ B) = d2x · B. V V ∂V

In R3, this can be written as Z Z dV ∇ ∧ B = dA nˆ ∧ B, V ∂V 110 multivector calculus.

which yields the divergence theorem after making a duality transformation B(x) = If(x), where f is a vector, by Z Z dV ∇ · f = dA nˆ · f, V ∂V

where nˆ is the normal speciﬁed by d2x = InˆdA, and d3x = IdV.

2.3.10 Divergence theorem.

Observe that for R3 we there are dot product relations in each of theorem 2.12, theorem 2.13 and theorem 2.14 which can be summarized as Theorem 2.15: Divergence theorem.

The divergence theorem may be generalized in R3 to multivectors M containing grades 0,1, or 2, but no grade 3 components Z Z dV ∇ · M = dA nˆ · M, V ∂V

where nˆ is the normal to the surface bounding V given by d2x = InˆdA.

2.4 multivector fourier transform and phasors.

It will often be convenient to utilize time harmonic (frequency domain) representations. This can be achieved by utilizing Fourier transform pairs or with a phasor representation. We may define Fourier transform pairs of multivector fields and sources in the conventional fashion Definition 2.8: Multivector Fourier transform pair.

The Fourier transform pair for a multivector function F(x, t) will be written as Z jωt F(x, t) = Fω(x)e dω 1 Z F (x) = F(x, t)e− jωtdt, ω 2π where j is an arbitrary scalar imaginary that commutes with all multivectors. 2.5 green’s functions. 111

In these transform pairs, the imaginary j need not be represented by any geometrical imagi- 3 nary such as e12. In particular, we need not assume that the representation of j is the R pseudoscalar I, despite the fact that I does commute with all R3 multivectors. We wish to have the freedom to assume that non-geometric real and imaginary operations can be performed without picking or leaving out any specific grade pseudoscalar components of the multivector fields or sources, so we won’t impose any a-priori restrictions on the representations of j. In particular, this provides the freedom to utilize phasor (fixed frequency) representations of our multivector functions. We will use the engineering convention for our phasor representations, where assuming a complex exponential time dependence of the following form is assumed Definition 2.9: Multivector phasor representation.

The phasor representation F(x) of a multivector valued (real) function F(x, t) is deﬁned implicitly as F(x, t) = Re F(x)e jωt ,

where j is an arbitrary scalar imaginary that commutes with all multivectors.

The complex valued multivector f (x) is still generated from the real Euclidean basis for R3, so there will be no reason to introduce complex inner products spaces into the mix. The reader must take care when reading any literature that utilizes Fourier transforms or phasor representation, since the conventions vary. In particular the physics representation of a phasor typically uses the opposite sign convention F(x, t) = Re F(x)e−iωt , which toggles the sign of all the imaginaries in derived results.

2.5 green’s functions.

2.5.1 Motivation.

Every engineer’s toolbox includes Laplace and Fourier transform tricks for transforming differential equations to the frequency domain. Here the space and time domain equivalent of the frequency and time domain linear system response function, called the Green’s function, is introduced. Everybody’s favorite diﬀerential equation, the harmonic oscillator, can be used as an illustrative example 00 0 2 x + kx + (ω0) x = f (t). (2.114)

Here derivatives are with respect to time, ω0 is the intrinsic angular frequency of the oscillator, k is a damping factor, and f (t) is a forcing function. If the oscillator represents a child on a 112 multivector calculus.

swing at the park (a pendulum system), then k represents the friction in the swing pivot and retardation due to wind, and the forcing function represents the father pushing the swing. The forcing function f (t) could include an initial impulse to get the child up to speed, or could have a periodic aspect, such as the father running underdogs6 as the child gleefully shouts “Again, again, again!” The full solution of this problem is x(t) = xs(t) + x0(t), where xs(t) is a solution of eq. (2.114) 00 0 2 and x0 is any solution of the homogeneous equation x0 + kx0 + (ω0) x0 = 0, picked to satisfy the boundary value constraints of the problem. Let’s attack this problem initially with Fourier transforms (deﬁnition 2.8) We can assume zero position and velocity for the non-homogeneous problem, since we can adjust the boundary conditions with the homogeneous solution x0(t). With zero boundary conditions on x, x0, the transform of eq. (2.114) is

2 2 ((− jω) + jω + (ω0) )X(ω) = F(ω), (2.115)

so the system is solved in the frequency domain by the system response function G(ω) X(ω) = G(ω)F(ω), (2.116)

where 1 G(ω) = − . (2.117) 2 2 ω − jω − (ω0) We can apply the inverse transformation to ﬁnd the time domain solution for the forced oscillator problem.

Z x(t) = dωG(ω)F(ω)e jωt Z Z ! 1 0 = dωG(ω) dt0 f (t0)e− jωt dt0 e jωt (2.118) 2π Z Z ! 1 0 = dt0 f (t0) dωG(ω)e jω(t−t ) . 2π

The frequency domain integral is the Green’s function. We’ll write this as Z 1 0 G(t, t0) = dωG(ω)e jω(t−t ). (2.119) 2π

6 The underdog is a non-passive swing pushing technique, where you run behind and under the swing, giving a push as you go. Before my kids learned to “pump their legs”, and even afterwards, this was their favorite way of being pushed on the swing. With two or more kids this forcing function tires quickly, as it is split between the oscillating children. 2.5 green’s functions. 113

If we can evaluate this integral, then the system can be considered solved, where a solution is given by the convolution integral Z 0 0 0 x(t) = dt f (t )G(t, t ) + x0(t). (2.120)

The Green’s function is the weighting factor that determines how much of f (t0) for each time t0 contributes to the motion of the system that is explicitly due to the forcing function. Green’s functions for physical problems are causal, so only forcing events in the past contribute to the current state of the system (i.e. if you were to depend on only future pushes of the swing, you would have a very bored child.) An alternate way of viewing a linear systems problem is to assume that a convolution solution of the form eq. (2.120) must exist. Since the equation is a linear, it is reasonable to assume that a linear weighted sum of all the forcing function values must contribute to the solution. If such a solution is assumed, then we can operate on that solution with the diﬀerential operator for the problem. For our harmonic oscillator problem that operator is

∂2 ∂ L = + k + (ω )2. (2.121) ∂t2 ∂t 0 We ﬁnd

! ∂2 ∂ f (t) = + k + (ω )2 x(t) ∂t2 ∂t 0 Z = dt0 f (t0)G(t, t0) (2.122) ! Z ∂2 ∂ = dt0 f (t0) + k + (ω )2 G(t, t0). ∂t2 ∂t 0

We see that the Green’s function, when acted on by the diﬀerential operator, must have the characteristics of a delta function ! ∂2 ∂ + k + (ω )2 G(t, t0) = δ(t − t0). (2.123) ∂t2 ∂t 0

The problem of determining the Green’s function, implicitly determining the solution of any forced system, can be viewed as seeking the solution of distribution equations of the form

LG(t, t0) = δ(t − t0). (2.124)

Framing the problem this way is independent of whatever techniques (transform or other) that we may choose to use to determine the structure of the Green’s function itself. Observe that the 114 multivector calculus.

Green’s function itself is not unique. In particular, we may add any solution of the homogeneous 0 problem LG0(t, t ) = 0 to the Green’s function, just as we can do so for the forced system itself. We will see that Green’s functions provide a general method of solving many of the linear diﬀerential equations that will be encountered in electromagnetism.

2.5.1.1 Time domain problems in electromagnetism

Examples of the PDEs that we can apply Green’s function techniques to include

! 1 ∂ ∇ + F(x, t) = J(x, t) (2.125a) c ∂t

! ! ! 1 ∂2 1 ∂ 1 ∂ ∇2 − F(x, t) = ∇ − ∇ + F(x, t) = B(x, t). (2.125b) c2 ∂t2 c ∂t c ∂t

The reader is no doubt familiar with the wave equation (eq. (2.125b)), where F is the waving function, and B is the forcing function. Scalar and vector valued wave equations are encountered in scalar and vector forms in conventional electromagnetism. We will see multivector variations of the wave equation, so it should be assumed that F and B are multivector valued. Equation (2.125a) is actually the geometric algebra form of Maxwell’s equation (singular), where F is a multivector with grades 1 and 2, and J is a multivector containing all the charge and current density contributions. We will call the operator in eq. (2.125a) the spacetime gradient7. Armed with Fourier transform or phasor representations, the frequency domain representations of eq. (2.125) are found to be

(∇ + jk) F(x) = J(x) (2.126a)

 ∇2 + k2 F(x) = (∇ − jk)(∇ + jk) F(x) = B(x), (2.126b)

where k = ω/c, and any explicit frequency dependence in our transform pairs has been suppressed. We will call these equations the first and second order Helmholtz equations respectively. The first order equation applies a multivector differential operator to a multivector field, which must equal the multivector forcing function (the sources).

7 A slightly diﬀerent operator is also called the spacetime gradient in STA (Space Time Algebra) [6], which employs a non-Euclidean basis to generate a four dimensional relativistic geometric algebra. Our spacetime gradient is related to the STA spacetime gradient by a constant factor. 2.5 green’s functions. 115

For statics problems (k = 0), we may work with real ﬁelds and sources, dispensing with any need to take real parts.

2.5.2 Green’s function solutions.

2.5.2.1 Unbounded.

The operators in eq. (2.125), and eq. (2.126) all have a similar linear structure. Abstracting that structure, all these problems have the form LF(x) = J(x), (2.127)

2 where L is an operator formed from a linear combination of linear operators 1, ∇, ∇ , ∂t, ∂tt. Given the linear structure of the PDE that we wish to solve, it makes sense to assume that the solutions also have a linear structure. The most general such solution we can assume has the form Z 0 0 0 0 0 0 F(x, t) = G(x, x ; t, t )J(x , t )dV dt + F0(x, t), (2.128)

0 0 where F0(x, t) is any solution to the equivalent homogeneous equation LF0 = 0, and G(x, x ; t, t ) is the Green’s function (to be determined) associated with eq. (2.127). Operating on the presumed solution eq. (2.128) with L yields

J(x, t) = LF(x, t) Z ! 0 0 0 0 0 0 = L G(x, x ; t, t )J(x , t )dV dt + F0(x, t) (2.129) Z = LG(x, x0; t, t0) J(x0, t0)dV0dt0, which shows that we require the Green’s function to have delta function semantics satisfying LG(x, x0; t, t0) = δ(x − x0)δ(t − t0). (2.130)

The scalar valued Green’s functions for the Laplacian and the (2nd order) Helmholtz equations are well known. The Green’s functions for the spacetime gradient and the 1st order Helmholtz equation (which is just the gradient when k = 0) are multivector valued and will be derived here. 116 multivector calculus.

2.5.2.2 Green’s theorem.

When the presumed solution is a superposition of only states in a bounded region then life gets a bit more interesting. For instance, consider a problem for which the differential operator is a function of space only, with a presumed solution such as Z 0 0 0 F(x) = dV B(x )G(x, x ) + F0(x), (2.131) V then life gets a bit more interesting. This sort of problem requires different treatment for operators that are first and second order in the gradient. For the second order problems, we require Green’s theorem, which must be generalized slightly for use with multivector fields. The basic idea is that we can relate the Laplacian of the Green’s function and the field F(x0) (∇0)2G(x, x0) = G(x, x0) (∇0)2F(x0) + ···. That relationship can be expressed as the integral of an antisymmetric sandwich of the two functions

Theorem 2.16: Green’s theorem

Given a multivector function F and a scalar function G Z Z F∇2G − G∇2F dV = (Fnˆ · ∇G − Gnˆ · ∇F) , V ∂V where ∂V is the boundary of the volume V.

A straightforward, but perhaps inelegant way of proving this theorem is to expand the antisymmetric product in coordinates

2 2 X F∇ G − G∇ F = F∂k∂kG − G∂k∂kF k X (2.132) = ∂k (F∂kG − G∂kF) − (∂kF)(∂kG) + (∂kG)(∂kF). k Since G is a scalar, the last two terms cancel, and we can integrate Z Z 2 2 X F∇ G − G∇ F dV = ∂k (F∂kG − G∂kF) . (2.133) V k V Each integral above involves one component of the gradient. From theorem 2.3 we know that Z Z ∇QdV = nˆ QdA, (2.134) V ∂V 2.5 green’s functions. 117 for any multivector Q. Equating components gives Z Z ∂kQdV = nˆ · ekQdA, (2.135) V ∂V which can be substituted into eq. (2.133) to ﬁnd Z Z 2 2 X F∇ G − G∇ F dV = nˆ · ek (F∂kG − G∂kF) dA V k ∂V Z (2.136) = (F(nˆ · ∇)G − G(nˆ · ∇)F) dA, ∂V which proves the theorem.

2.5.2.3 Bounded solutions to ﬁrst order problems.

For ﬁrst order problems we will need an intermediate result similar to Green’s theorem. Lemma 2.1: Normal relations for a gradient sandwich.

Given multivector functions F(x0), G(x, x0), and a gradient ∇0 acting bidirectionally on functions of x0, we have

Z ←0! Z →0 ! Z − G(x, x0) ∇ F(x0)dV0 = G(x, x0) ∇ F(x0) dV0 − G(x, x0)nˆ 0F(x0)dA0. V V ∂V

This follows directly from theorem 2.3

Z Z ↔0 G(x, x0)nˆ 0F(x0)dA0 = G(x, x0) ∇ F(x0)dV0 ∂V V (2.137) Z ←0! Z →0 ! = G(x, x0) ∇ F(x0)dV0 + G(x, x0) ∇ F(x0) dV0, V V which can be rearranged to prove lemma 2.1.

2.5.3 Helmholtz equation.

2.5.3.1 Unbounded superposition solutions for the Helmholtz equation.

The specialization of eq. (2.130) to the Helmholtz equation eq. (2.126b) is ∇2 + k2 G(x, x0) = δ(x − x0). (2.138) While it is possible [20] to derive the Green’s function using Fourier transform techniques, we will state the result instead, which is well known 118 multivector calculus.

Theorem 2.17: Green’s function for the Helmholtz operator.

The advancing (causal), and the receding (acausal) Green’s functions satisfying eq. (2.138) are respectively

0 e− jkkx−x k G (x, x0) = − adv 4π kx − x0k 0 e jkkx−x k G (x, x0) = − . rec 4π kx − x0k

We will use the advancing (causal) Green’s function, and refer to this function as G(x, x0) without any subscript. Because it may not be obvious that these Green’s function representations are valid in a multivector context, a demonstration of this fact can be found in appendix C.1. Observe that as a special case, the Helmholtz Green’s function reduces to the Green’s function for the Laplacian when k = 0 1 G(x, x0) = − . (2.139) 4π kx − x0k

2.5.3.2 Bounded superposition solutions for the Helmholtz equation.

For our application of theorem 2.17 to the Helmholtz problem, we are actually interested in a antisymmetric sandwich of the Helmholtz operator by the function F and the scalar (Green’s) function G, but that reduces to an asymmetric sandwich of our functions around the Laplacian

 ¨ ¨ ∇2 2 − ∇2 2 ∇2 ¨2 − ∇2 − ¨2 F + k G G + k F = F G + ¨Fk G G F ¨Gk F (2.140) = F∇2G − G∇2F,

so Z Z F(x0) (∇0)2 + k2 G(x, x0) = G(x, x0) (∇0)2 + k2 F(x0)dV0 V VZ 0 0 0 0 0 0 0 0 0 + F(x )(nˆ · ∇ )G(x, x ) − G(x, x )(nˆ · ∇ )F(x ) dA . ∂V (2.141) 2.5 green’s functions. 119

This shows that if we assume the Green’s function satisﬁes the delta function condition eq. (2.138) , then the general solution of eq. (2.126b) is formed from a bounded superposition of sources is Z F(x) = G(x, x0)B(x0)dV0 V Z (2.142) + (G(x, x0)(nˆ 0 · ∇0)F(x0) − F(x0)(nˆ 0 · ∇0)G(x, x0)) dA0. ∂V

We are also free to add in any speciﬁc solution F0(x) that satisﬁes the homogeneous Helmholtz equation. There is also freedom to add any solution of the homogeneous Helmholtz equation to the Green’s function itself, so it is not unique. For a bounded superposition we generally desire that the solution F and its normal derivative, or the Green’s function G (and it’s normal derivative) or an appropriate combination of the two are zero on the boundary, so that the surface integral is killed.

2.5.4 First order Helmholtz equation.

The specialization of eq. (2.130) to the ﬁrst order Helmholtz equation eq. (2.126a) is (∇ + jk) G(x, x0) = δ(x − x0). (2.143)

This Green’s function is multivector valued Theorem 2.18: Green’s function for the ﬁrst order Helmholtz operator.

The Green’s function for the ﬁrst order Helmholtz operator ∇ + jk satisﬁes

→ ←0 ! ∇ + jk G(x, x0) = G(x, x0) − ∇ + jk = δ(x − x0),

and has the value ! e− jkr rˆ G(x, x0) = jk (1 + rˆ) + , 4πr r

where r = x − x0, r = krk and rˆ = r/r, and ∇0 denotes diﬀerentiation with respect to x0.

A special but important case is the k = 0 condition, which provides the Green’s function for the gradient, which is vector valued

1 rˆ G(x, x0; k = 0) = . (2.144) 4π r2 120 multivector calculus.

If we denote the (advanced) Green’s function for the 2nd order Helmholtz operator theorem 2.17 as φ(x, x0), we must have

→ → → ∇ + jk G(x, x0) = δ(x − x0) = ∇ + jk ∇ − jk φ(x, x0), (2.145)

we see that the Green’s function is given by

→ G(x, x0) = ∇ − jk φ(x, x0). (2.146)

This can be computed directly

! → e− jkr G(x, x0) = ∇ − jk − 4πr ! ! ∂ e− jkr = rˆ − jk − ∂r 4πr ! ! (2.147) −e− jkr jk 1 jk = rˆ − − − 4π r r2 r ! e− jkr rˆ = jk (1 + rˆ) + , 4π r

as claimed. Observe that since φ is scalar valued, we can also rewrite eq. (2.146) in terms of a right acting operator

← G(x, x0) = φ(x, x0) ∇ − jk

←0 ! (2.148) = φ(x, x0) − ∇ − jk ,

←0 ! ←0 ! G(x, x0) − ∇ + jk = φ(x, x0) (∇ )2 + k2 = δ(x − x0). (2.149)

This is relevant for bounded superposition states, which we will discuss next now that the R 0 0 0 proof of theorem 2.18 is complete. In particular addition of V G(x, x ) jkF(x )dV to both sides of lemma 2.1 gives

Z ←0 !! Z →0 ! ! G(x, x0) − ∇ + jk F(x0)dV0 = G(x, x0) ∇ + jk F(x0) dV0 V V Z (2.150) − G(x, x0)nˆ 0F(x0)dA0. ∂V 2.5 green’s functions. 121

Utilizing theorem 2.18, and substituting J(x0) from eq. (2.126a), we ﬁnd that one solution to the ﬁrst order Helmholtz equation is Z Z F(x) = G(x, x0)J(x0)dV0 − G(x, x0)nˆ 0F(x0)dA0. (2.151) V ∂V

We are free to add any speciﬁc solution F0 that satisﬁes the homogeneous equation (∇ + jk) F0 = 0.

2.5.5 Spacetime gradient.

We want to ﬁnd the Green’s function that solves spacetime gradient equations of the form eq. (2.125a). For the wave equation operator, it is helpful to introduce a d’Lambertian operator, deﬁned as follows.

Deﬁnition 2.10: d’Lambertian (wave equation) operator.

The symbol is used to represent the d’Lambertian (wave equation) operator, with a positive sign on the Laplacian term ! ! 1 ∂ 1 ∂ 1 ∂2 = ∇ − ∇ + = ∇2 − . c ∂t c ∂t c2 ∂t2

We will be able to derive the Green’s function for the spacetime gradient from the Green’s function for the d’Lambertian. The Green’s function for the spacetime gradient is multivector valued and given by the following.

Theorem 2.19: Green’s function for the spacetime gradient.

The Green’s function for the spacetime gradient ∇ + (1/c)∂t satisﬁes ! 1 ∂ ∇ + G(x − x0, t − t0) = δ(x − x0)δ(t − t0), c ∂t

and has the value ! 1 rˆ ∂ rˆ 1 ∂ G(x − x0, t − t0) = − + + δ(−r/c + t − t0), 4π r2 ∂r r cr ∂t

where r = x − x0, r = krk and rˆ = r/r. 122 multivector calculus.

With the help of eq. (C.18) it is possible to further evaluate the delta function derivatives, however, we will defer doing so until we are ready to apply this Green’s function in a convolution integral to solve Maxwell’s equation. To prove this result, let φ(x − x0, t − t0) be the retarded time (causal) Green’s function for the wave equation, satisfying ! ! 1 ∂ 1 ∂ φ(x − x0, t − t0) = ∇ + ∇ − φ(x − x0, t − t0) c ∂t c ∂t (2.152) = δ(x − x0)δ(t − t0).

This function has the value 1 φ(r, t − t0) = − δ(−r/c + t − t0), (2.153) 4πr where r = x − x0, r = krk. Derivations of this Green’s function, and it’s acausal advanced time friend, can be found in [20], [14], and use the usual Fourier transform and contour integration tricks. Comparing eq. (2.152) to the deﬁning statement of theorem 2.19, we see that the spacetime gradient Green’s function is given by ! 1 ∂ G(x − x0, t − t0) = ∇ − φ(r, t − t0) c ∂t ! (2.154) ∂ 1 ∂ = rˆ − φ(r, t − t0), ∂r c ∂t

where rˆ = r/r. Evaluating the derivatives gives ! 1 ∂ 1 ∂ δ(−r/c + t − t0) G(r, t − t0) = − rˆ − 4π ∂r c ∂t r (2.155)! 1 rˆ ∂ rˆ 1 ∂ = − δ(−r/c + t − t0) − δ(−r/c + t − t0) − δ(−r/c + t − t0) , 4π r ∂r r2 cr ∂t which completes the proof after some sign cancellation and minor rearrangement.

2.6 helmholtz theorem.

In conventional electromagnetism Maxwell’s equations are posed in terms of separate divergence and curl equations. It is therefore desirable to show that the divergence and curl of a function and it’s normal characteristics on the boundary of an integration volume determine that function uniquely. This is known as the Helmholtz theorem 2.6 helmholtz theorem. 123

Theorem 2.20: Helmholtz ﬁrst theorem.

A vector M is uniquely determined by its divergence

∇ · M = s,

and curl

∇ × M = C,

and its value over the boundary.

The conventional proof of Helmholtz’s theorem uses the Green’s function for the (second order) Helmholtz operator. Armed with a vector valued Green’s function for the gradient, a ﬁrst order proof is also possible. As illustrations of the geometric integration theory developed in this chapter, both strategies will be applied here to this problem. In either case, we start by forming an even grade multivector (gradient) equation containing both the dot and cross product contributions

∇M = ∇ · M + I∇ × M = s + IC. (2.156)

First order proof. For the ﬁrst order case, we perform a grade one selection of lemma 2.1, setting F = M where G is the Green’s function for the gradient given by eq. (2.144). The proof follows directly

Z ←0! M(x) = − G(x, x0) ∇ M(x0)dV0 V Z * →0 !+ Z 0 0 0 0 0 0 0 = G(x, x ) ∇ M(x ) dV − G(x, x )nˆ M(x ) 1dA V 1 ∂V Z 1 = (x − x0) s(x0) + IC(x0) dV0 0 3 1 V 4π kx − x k Z (2.157) 1 0 0 0 0 − (x − x )nˆ M(x ) dA 0 3 1 ∂V 4π kx − x k Z 1 = (x − x0)s(x0) − (x − x0) × C(x0) dV0 0 3 V 4π kx − x k Z 1 0 0 0 0 − (x − x )nˆ M(x ) dA . 0 3 1 ∂V 4π kx − x k 124 multivector calculus.

If M is well behaved enough that the boundary integral vanishes on an inﬁnite surface, we see that M is completely speciﬁed by the divergence and the curl. In general, the divergence and the curl, must also be supplemented by the the value of vector valued function on the boundary. Observe that the boundary integral has a particularly simple form for a spherical surface or radius R centered on x0. Switching to spherical coordinates r = x0 − x = R rˆ(θ, φ) where rˆ = (x0 − x)/kx0 − xk is the outwards normal, we have

Z Z 0 1 0 0 0 0 M(x ) 0 − (x − x )nˆ M(x ) dA = dA k − 0k3 1 k − 0k2 ∂V 4π x x ∂V 4π x x (2.158) 1 Z π Z 2π = M(R, θ, φ) sin θdθdφ. 4π θ=0 φ=0 This is an average of M over the surface of the radius-R sphere surrounding the point x where the ﬁeld M is evaluated.

Second order proof. Again, we use eq. (2.156) to discover the relation between the vector M and its divergence and curl. The vector M can be expressed at the point of interest as a convolution with the delta function at all other points in space Z M(x) = dV0δ(x − x0)M(x0). (2.159) V

The Laplacian representation of the delta function in R3 is 1 1 δ(x − x0) = − ∇2 , (2.160) 4π kx − x0k so M can be represented as the following convolution 1 Z 1 0∇2 0 M(x) = − dV 0 M(x ). (2.161) 4π V kx − x k 2.6 helmholtz theorem. 125

Using this relation and proceeding with a few applications of the chain rule, plus the fact that ∇1/kx − x0k = −∇01/kx − x0k, we ﬁnd

Z 1 −4πM(x) = dV0∇2 M(x0) kx − x0k * V + Z 1 0∇2 0 = dV 0 M(x ) V kx − x k * ! 1 + Z 1 0∇ ∇0 0 = − dV 0 M(x ) V kx − x k * 1 !+ (2.162) Z M(x0) ∇0M(x0) ∇ 0 ∇0 = − dV 0 − 0 V kx − x k kx − x k * + * 1 + Z M(x0) Z s(x0) + IC(x0) ∇ 0 ∇ 0 = − dA nˆ 0 + dV 0 ∂V kx − x k V kx − x k * +1 1 Z M(x0) Z s(x0) Z IC(x0) ∇ 0 ∇ 0 ∇ 0 = − dA nˆ 0 + dV 0 + · dV 0 . ∂V kx − x k 1 V kx − x k V kx − x k By inserting a no-op grade selection operation in the second step, the trivector terms that would show up in subsequent steps are automatically filtered out. This leaves us with a boundary term dependent on the surface and the normal and tangential components of M. Added to that is a pair of volume integrals that provide the unique dependence of M on its divergence and curl. When the surface is taken to infinity, which requires kMk /kx − x0k → 0, then the dependence of M on its divergence and curl is unique. In order to express final result in traditional vector algebra form, a couple transformations are required. The first is that

2 haIbi1 = I a × b = −a × b. (2.163)

For the grade selection in the boundary integral, note that

h∇nXˆ i1 = h∇(nˆ · X)i1 + h∇(nˆ ∧ X)i1 = ∇(nˆ · X) + h∇I(nˆ × X)i1 (2.164) = ∇(nˆ · X) − ∇ × (nˆ × X).

These give

1 Z M(x0) 1 Z M(x0) M(x) = ∇ dA0nˆ · − ∇ × dA0nˆ × 4π kx − x0k 4π kx − x0k ∂V ∂V (2.165) 1 Z s(x0) 1 Z C(x0) ∇ 0 ∇ 0 − dV 0 + × dV 0 . 4π V kx − x k 4π V kx − x k 126 multivector calculus.

2.7 problem solutions.

Answer for Exercise 2.1 Assuming the representation of eq. (2.10), the dot products are

1 2 1 = x1 · x = ax1 + bx1 · x2 1 2 0 = x2 · x = ax2 · x1 + bx2 2 2 (2.22) 0 = x1 · x = cx1 + dx1 · x2 2 2 1 = x2 · x = cx2 · x1 + dx2. This can be written out as a pair of matrix equations       2 1  x x1 · x2 a   =  1       2    0 x2 · x1 x2 b       (2.23) 2 0  x x1 · x2 c   =  1    .    2    1 x2 · x1 x2 d The matrix inverse is  −1   2 2  x x1 · x2 1  x −x1 · x2  1  =  2  . (2.24)  2  x2x2 − (x · x )2  2  x2 · x1 x2 1 2 1 2 −x2 · x1 x1 Multiplying by the (1, 0), and (0, 1) vectors picks out the respective columns, and gives eq. (2.11).

Answer for Exercise 2.2 The bivector for the plane spanned by this basis is

x1 ∧ x2 = (e1 + 2e2) ∧ (e2 − e3) = e12 − e13 − 2e23 (2.26) = e12 + e31 + 2e32.

This has the square

2 (x1 ∧ x2) = (e12 + e31 + 2e32) · (e12 + e31 + 2e32) = −1 − 1 − 4 (2.27) = −6. 2.7 problem solutions. 127

Dotting −x1 with the bivector is

x1 · (x2 ∧ x1) = − (e1 + 2e2) · (e12 + e31 + 2e32) = − (e2 − e3 − 2e1 − 4e3) (2.28) = 2e1 − e2 + 5e3.

For x2 the dot product with the bivector is

x2 · (x1 ∧ x2) = (e2 − e3) · (e12 + e31 + 2e32) = −e1 − 2e3 − e1 − 2e2 (2.29) = −2e1 − 2e2 − 2e3, so

1 1 x = (e1 + e2 + e3) 3 (2.30) 1 x2 = (−2e + e − 5e ) . 6 1 2 3 It is easy to verify that this has the desired semantics.

Answer for Exercise 2.4 iφ Computing the various dot products is made easier by noting that e3 and e commute, jθ − jθ iφ −iφ iφ −iφ whereas e e3 = e3e , e1e = e e1, e2e = e e2 (since e3 j, e1i and e2i all anticommute)

D jθ iφ jθE xr · xθ = e3e e1e e D jθ jθ iφE = e e3e e1e D − jθ jθ iφE (2.74a) = e3e e e1e D iφE = e3e1e = 0

D jθ iφE xr · xφ = e3e r sin θe2e D iφ iφE = r sin θ e3 cos θ + e31 sin θe e2e 2 D iφ iφE (2.74b) = r sin θ e1e e2e 2 = r sin θhe1e2i = 0 128 multivector calculus.

D iφ jθ iφE xθ · xφ = r sin θ e1e e e2e D jθE = r sin θ e2e1e D iφE (2.74c) = r sin θ e2e1 cos θ + e31 sin θe 2 D iφE = r sin θ e32e = 0.

Answer for Exercise 2.5 Using the commutation relations from last problem, ﬁrst note that

iφ jθ iφ −iφ iφ e1e e = e1 cos θe + sin θe31e e −iφ iφ = e1 cos θ + sin θe31e e (2.75) iφ iφ = cos θ − sin θe31e e1e − jθ iφ = e e1e .

This gives

D jθ iφ jθ iφE D iφ iφE e3e e1e e e2e = e3e1e e2e 3 3 (2.76) = he3e1e2i3 = e123. ELECTROMAGNETISM. 3

3.1 conventional formulation.

Maxwell’s equations provide an abstraction, the field, that aggregates the effects of an arbitrary electric charge and current distribution on a “test” charge distribution. The test charge is assumed to be small and isolated enough that it does not also appreciably change the fields themselves. Once the fields are determined, the Lorentz force equation can be used to determine the dynamics of the test particle. These dynamics can be determined without having to compute all the interactions of that charge with all the charges and currents in space, nor having to continually account for the interactions of those charge with each other. We will use vector differential form of Maxwell’s equations with antenna theory extensions (fictitious magnetic sources) as our starting point ∂B ∇ × E = −M − (3.1a) ∂t

∂D ∇ × H = J + (3.1b) ∂t

∇ · D = ρ (3.1c)

∇ · B = ρm. (3.1d)

These equations relate the primary electric and magnetic ﬁelds

• E(x, t) : Electric ﬁeld intensity [V/m] (Volts/meter)

• H(x, t) : Magnetic ﬁeld intensity [A/m] (Amperes/meter),

and the induced electric and magnetic ﬁelds

• D(x, t) : Electric ﬂux density (or displacement vector) [C/m] (Coulombs/meter)

• B(x, t) : Magnetic ﬂux density [W/m2] (Webers/square meter),

to the charge densities

129 130 electromagnetism.

• ρ(x, t) : Electric charge density [C/m3] (Coulombs/cubic meter)

3 • ρm(x, t) : Magnetic charge density [W/m ] (Webers/cubic meter),

and the current densities

• J(x, t) : Electric current density [A/m2] (Amperes/square meter),

• M(x, t) : Magnetic current density [V/m2] (Volts/square meter).

All of the fields and sources can vary in space and time, and are specified here in SI units. The sources M, ρm can be considered fictional, representing physical phenomena such as infinitesimal current loops. In general, the relationship between the electric and magnetic fields (constitutivity relationships) may be complicated non-isotropic tensor operators, functions of all of E, D, B and H. In this book, we will assume that the constitutive relationships between the electric and magnetic fields are independent B = µH (3.2a)

D = E, (3.2b)

where = r0 is the permittivity of the medium [F/m] (Farads/meter), and µ = µrµ0 is the permeability of the medium [H/m] (Henries/meter). The permittivity and permeability may be functions of both time and position, and model the materials that the ﬁelds are propagating through. In free space µr = 1 and r = 1 so these relationships are simply

B = µ0H (3.3a)

D = 0E, (3.3b)

where

−12 2 2 • 0 = 8.85 × 10 C /N/m : Permittivity of free space (Coulombs squared/Newton/square meter)

−7 2 • µ0 = 4π × 10 N/A : Permeability of free space (Newtons/Ampere-squared). 3.1 conventional formulation. 131

8 2 These constants are related to the speed of light, c = 3.00 × 10 m/s by µ00 = 1/c . Antenna theory extends Maxwell’s equations with fictional magnetic charge and current densities that are useful to model real phenomena such as infinitesimal current loops. Antenna related problems are usually tackled in the frequency domain. We will use the engineering conventions for the frequency domain described in section 2.4. Continuous models for charge and current distributions are used in Maxwell’s equations, despite the fact that charges (i.e. electrons) are particles, and are not distributed in space. The discrete nature of electronic charge can be modelled using a delta function representation of the charge and current densities X ρ(x, t) = qaδ(x − xa(t)) a X (3.4) J(x, t) = qava(x, t). a This model is inherently non-quantum mechanical, as it assumes that it is possible to simul- taneous measure the position and velocity of an electron. The dynamics of particle interaction with the fields are provided by the Lorentz force and power equations dp = q (E + v × B) (3.5a) dt

dE = qE · v. (3.5b) dt Both the energy and the momentum relations of eq. (3.5) are stated, since the simplest (relativistic) form of the Lorentz force equation directly encodes both. For readers unfamiliar with eq. (3.5b), exercise 3.1 provides a derivation method. The quantities involved in the Lorentz equations are

• p(x, t) : Test particle momentum [kg m/s] (Kilogram meters/second)

• E(x, t) : Test particle kinetic energy [J] (Joules, kilogram meter^2/second^2)

• q : Test particle charge [C] (Coulombs)

• v : Test particle velocity [m/s] (Meters/second)

The task of extracting all the physical meaning from the Maxwell and Lorentz equations is a diﬃcult one. Our attempt to do so will use the formalism of geometric algebra. 132 electromagnetism.

3.1.1 Problems.

Exercise 3.1 Lorentz power and force relationship. (§17 [17]) Using the relativistic deﬁnitions of momentum and energy mv p(x, t) = p 1 − v2/c2 mc2 E(x, t) = p , 1 − v2/c2

show that dE/dt = v · dp/dt, and use this to derive eq. (3.5b) from eq. (3.5a).

3.2 maxwell’s equation.

We will work with a multivector representation of the fields in isotropic media satisfying the constituency relationships from eq. (3.2), and define a multivector field that includes both electric and magnetic components

Deﬁnition 3.1: Electromagnetic ﬁeld strength.

The electromagnetic ﬁeld strength ([V/m] (Volts/meter)) is deﬁned as

F = E + IηH (= E + IcB),

where p • η = µ/ ([Ω] Ohms), is the impedance of the media. √ • c = 1/ µ ([m/s] meters/second), is the group velocity of a wave in the media. When = 0, µ = µ0, c is the speed of light.

F is called the Faraday by some authors.

The factors of η (or c) that multiply the magnetic fields are for dimensional consistency, √ √ √ since [ E] = [ µH] = [B/ µ]. The justification for imposing a dual (or complex) structure on the electromagnetic field strength can be found in the historical development of Maxwell’s equations, but we will also see such a structure arise naturally in short order. 3.2 maxwell’s equation. 133

No information is lost by imposing the complex structure of definition 3.1, since we can always obtain the electric field vector E and the magnetic field bivector IH by grade selection from the electromagnetic field strength when desired

E = hFi1 1 (3.6) IH = hFi . η 2 We will also deﬁne a multivector current containing all charge densities and current densities

Deﬁnition 3.2: Multivector current.

The current ([A/m2] (Amperes/square meter)) is deﬁned as

J = η (cρ − J) + I (cρm − M) .

When the ﬁctitious magnetic source terms (ρm, M) are included, the current has one grade for each possible source (scalar, vector, bivector, trivector). With only conventional electric sources, the current is still a multivector, but contains only scalar and vector grades. Given the multivector ﬁeld and current, it is now possible to state Maxwell’s equation (singular) in its geometric algebra form

Theorem 3.1: Maxwell’s equation.

Maxwell’s equation is a multivector equation relating the change in the electromagnetic ﬁeld strength to charge and current densities and is written as ! 1 ∂ ∇ + F = J. c ∂t

Maxwell’s equation in this form will be the starting place for all the subsequent analysis in this book. As mentioned in section 2.5, the operator ∇ + (1/c)∂t will be called the spacetime gradient1.

1 This form of spacetime gradient is given a special symbol by a number of authors, but there is no general agreement on what to use. Instead of entering the ﬁght, it will be written out in full in this book. 134 electromagnetism.

To prove theorem 3.1 we first insert the isotropic constituency relationships from eq. (3.2) into eq. (3.1), so that we are working with two field variables instead of four 1 ∇ · E = ρ ∂H ∇ × E = −M − µ ∂t 1 (3.7) ∇ · H = ρ µ m ∂E ∇ × H = J + ∂t Inserting a = ∇ into eq. (1.62) the vector product of the gradient with another vector ∇b = ∇ · b + I∇ × b. (3.8) The dot and cross products for E and H in eq. (3.7) can be grouped using eq. (3.8) into multivector gradient equations ! 1 ∂H ∇E = ρ + I −M − µ ∂t ! (3.9) 1 ∂E ∇H = ρ + I J + . µ m ∂t Multiplying the gradient equation for the magnetic field by ηI so that both equations have the same dimensions, and so that the electric field appears in both equations as E and not IE, we find 1 ∂ 1 ∇E + (IηH) = ρ − IM c ∂t (3.10) 1 ∂E ∇IηH + = Icρ − ηJ, c ∂t m where µ/η = η = 1/c was used to simplify things slightly, and all the field contributions have been moved to the left hand side. The first multivector equation has only scalar and bivector grades, whereas the second has only vector and trivector grades. This means that if we add these equations, we can recover each by grade selection, and no information is lost. That sum is ! 1 ∂ ∇ + (E + IηH) = η (cρ − J) + I (cρ − M) . (3.11) c ∂t m Application of definition 3.1 and definition 3.2 to eq. (3.11) proves the theorem, verifying the assertion that Maxwell’s equations can be consolidated into a single multivector equation. There is a lot of information packed into this single equation. Where possible, we want to work with the multivector form of Maxwell’s equation, either in the compact form of theorem 3.1 or the explicit form of eq. (3.11), and not decompose Maxwell’s equation into the conventional representation by grade selection operations. 3.3 wave equation and continuity. 135

3.2.0.1 Problems.

Exercise 3.2 Dot and cross product relation to vector product. Using coordinate expansion, convince yourself of the validity of eq. (3.8).

Exercise 3.3 Extracting the conventional Maxwell’s equations. Apply grade 0,1,2, and 3 selection operations to eq. (3.11). Determine the multiplicative (scalar or trivector) constants required to obtain eq. (3.7) from the equations that result from such grade selection operations.

3.3 wave equation and continuity.

Some would argue that the conventional form eq. (3.1a) of Maxwell’s equations have built in redundancy since continuity equations on the charge and current densities couple some of these equations. We will take an opposing view, and show that such continuity equations are necessary consequences of Maxwell’s equation in its wave equation form, and derive those conditions. This amounts to a statement that the multivector current J is not completely unconstrained.

Theorem 3.2: Electromagnetic wave equation and continuity conditions.

The electromagnetic ﬁeld is a solution to the non-homogeneous wave equation ! 1 ∂ F = ∇ − J. c ∂t

In source free conditions, this reduces to a homogeneous wave equation, with group velocity c, the speed of the wave in the media. When expanded explicitly in terms of electric and magnetic ﬁelds, and charge and current densities, this single equation resolves to a non-homogeneous wave equation for each of the electric and magnetic ﬁelds

1 ∂J E = ∇ρ + µ + ∇ × M ∂t 1 ∂M H = ∇ρ + − ∇ × J, µ m ∂t 136 electromagnetism.

as well as a pair of continuity equations coupling the respective charge and current densities ∂ρ ∇ · J + = 0 ∂t ∂ρ ∇ · M + m = 0. ∂t

To prove, we operate on theorem 3.1 with ∇ − (1/c)∂t, one of the factors, along with the spacetime gradient, of the d’Lambertian (wave equation) operator, which gives ! 1 ∂ F = ∇ − J. (3.12) c ∂t

Since the left hand side has only grades 1 and 2, eq. (3.12) splits naturally into two equations, one for grades 1,2 and one for grades 0,3 * ! + 1 ∂ F = ∇ − J c ∂t 1,2 * ! + (3.13) 1 ∂ 0 = ∇ − J . c ∂t 0,3 Unpacking these further, we ﬁnd that there is information carried in the requirement that the grade 0,3 selection of eq. (3.13) is zero. In particular, grade 0 selection gives

0 = h(∇ − (1/c)∂t)Ji * + 1 ∂ = ∇ − (η (cρ − J) + I (cρ − M)) c ∂t m (3.14) ! ∂ρ = −η ∇ · J + , ∂t

which demonstrates the continuity condition on the electric sources. Similarly, grade three selection gives

0 = h(∇ − (1/c)∂t)Ji * 3 + 1 ∂ = ∇ − (η (cρ − J) + I (cρ − M)) c ∂t m (3.15) ! 3 ∂ρ = −I ∇ · M + m , ∂t

which demonstrates the continuity condition on the (ﬁctitious) magnetic sources if included in the current. 3.4 plane waves. 137

For the non-homogeneous wave equation of theorem 3.2, the current derivatives may be expanded explicitly. For the wave equation for the electric ﬁeld, this is

* ! + 1 ∂ E = ∇ − J c ∂t * ! 1 + 1 ∂ ρ = ∇ − − ηJ + I (cρm − M) c ∂t 1 1 1 ∂J = ∇ρ − I (∇ ∧ M) + η (3.16) c ∂t * ! + 1 ∂ = ∇ − J c ∂t 1 1 ∂J = ∇ρ + µ + ∇ × M, ∂t as claimed. The forced magnetic ﬁeld equation is

* ! + 1 1 ∂ H = ∇ − J ηI c ∂t * ! 2 + 1 1 ∂ ρ = ∇ − − ηJ + I (cρ − M) ηI c ∂t m ! 2 1 I ∂M = −∇ ∧ J + Ic∇ρ + (3.17) ηI m c ∂t ! 1 1 ∂M = −I (∇ × J) + I ∇ρ + I I µ m ∂t 1 ∂M = ∇ρ + − ∇ × J, µ m ∂t completing the proof.

3.4 plane waves.

With all sources zero, the free space Maxwell’s equation as given by theorem 3.1 for the electromagnetic ﬁeld strength reduces to just ! 1 ∂ ∇ + F(x, t) = 0. (3.18) c ∂t

Utilizing a phasor representation of the form definition 2.9, we will define the phasor representation of the field as 138 electromagnetism.

Deﬁnition 3.3: Plane wave.

We represent the electromagnetic ﬁeld strength plane wave solution of Maxwell’s equation in phasor form as F(x, t) = Re F(k)e jωt ,

where the complex valued multivector F(k) also has a presumed exponential dependence

F(k) = Fe˜ − jk·x.

We will now show that solutions of the electromagnetic ﬁeld wave equation have the form

Theorem 3.3: Plane wave solutions to Maxwell’s equation.

Single frequency plane wave solutions of Maxwell’s equation have the form F(x, t) = Re 1 + kˆ kˆ ∧ E e− jk·x+ jωt ,

where kkk = ω/c, kˆ = k/kkk is the unit vector pointing along the propagation direction, and E is any complex-valued vector variable. When a E · k = 0 constraint is imposed on the vector variable E, that variable can be interpreted as the electric ﬁeld, and the solution reduces to F(x, t) = Re 1 + kˆ E e− jk·x+ jωt ,

showing that the ﬁeld phasor F(k) = E(k) + IηH(k) splits naturally into electric and magnetic components

E(k) = E e− jk·x ηH(k) = kˆ × E e− jk·x,

where the directions kˆ, E, H form a right handed triple. 3.4 plane waves. 139

− jk·x+ jωt We wish to act on F(k)e with the spacetime gradient ∇ + (1/c)∂t, but must take care of order when applying the gradient to a non-scalar valued function. In particular, if A is a multivector, then

3 − jk·x X − jk·x ∇Ae = em∂mAe m=1 3 (3.19) X − jk·x = emA (− jkm) e m=1 = − jkA.

Therefore, insertion of the presumed phasor solution of the ﬁeld from deﬁnition 3.3 into eq. (3.18) gives ω 0 = − j k − F(k). (3.20) c If F(k) has a left multivector factor ω F(k) = k + F˜, (3.21) c where F˜ is a multivector to be determined, then

ω ω ω k − F(k) = k − k + F˜ c c c ! (3.22) ω2 = k2 − F˜, c which is zero if if kkk = ω/c. Let kkk F˜ = F0 + F1 + F2 + F3, where F0, F1, F2, and F3 respectively have grades 0,1,2,3, so that

F(k) = 1 + kˆ (F0 + F1 + F2 + F3) = F0 + F1 + F2 + F3 + kˆ F0 + kˆ F1 + kˆ F2 + kˆ F3 (3.23) = F + F + F + F + kˆ F + kˆ · F + kˆ · F + kˆ · F + kˆ ∧ F + kˆ ∧ F 0 1 2 3 0 1 2 3 1 2 = F0 + kˆ · F1 + F1 + kˆ F0 + kˆ · F2 + F2 + kˆ · F3 + kˆ ∧ F1 + F3 + kˆ ∧ F2 .

Since the ﬁeld F has only vector and bivector grades, the grades zero and three components of the expansion above must be zero, or

F0 = −kˆ · F1 (3.24) F3 = −kˆ ∧ F2, 140 electromagnetism.

 F(k) = 1 + kˆ F1 − kˆ · F1 + F2 − kˆ ∧ F2 (3.25) = 1 + kˆ F1 − kˆ F1 + kˆ ∧ F1 + F2 − kˆ F2 + kˆ · F2 .

The multivector 1 + kˆ has the projective property of gobbling any leading factors of kˆ

(1 + kˆ)kˆ = kˆ + 1 (3.26) = 1 + kˆ,

so for Fi ∈ F1, F2

(1 + kˆ)(Fi − kˆ Fi) = (1 + kˆ)(Fi − Fi) = 0, (3.27)

leaving F(k) = 1 + kˆ kˆ · F2 + kˆ ∧ F1 . (3.28)

For kˆ · F2 to be non-zero F2 must be a bivector that lies in a plane containing kˆ, and kˆ · F2 is a vector in that plane that is perpendicular to kˆ. On the other hand kˆ ∧ F1 is non-zero only if F1 has a non-zero component that does not lie in along the kˆ direction, but kˆ ∧ F1, like F2 describes a plane that containing kˆ. This means that having both bivector and vector free variables F2 and F1 provide more degrees of freedom than required. For example, if E is any vector, and F2 = kˆ ∧ E, then 1 + kˆ kˆ · F2 = 1 + kˆ kˆ · kˆ ∧ E = 1 + kˆ E − kˆ kˆ · E (3.29) = 1 + kˆ kˆ kˆ ∧ E = 1 + kˆ kˆ ∧ E, which has the form 1 + kˆ kˆ ∧ F1 , so the electromagnetic ﬁeld strength phasor may be generally written F(k) = 1 + kˆ kˆ ∧ E e− jk·x, (3.30) Expanding the multivector factor 1 + kˆ kˆ ∧ E we ﬁnd

 1 + kˆ kˆ ∧ E = kˆ · kˆ ∧ E + kˆ ∧ kˆ ∧ E + kˆ ∧ E (3.31) = E − kˆ kˆ ∧ E + kˆ ∧ E. 3.5 statics. 141

The vector grade has the component of E along the propagation direction removed (i.e. it is the rejection), so there is no loss of generality should a E · k = 0 constraint be imposed. Such as constraint let’s us write the bivector as a vector product kˆ ∧ E = kEˆ , and then use the projective property eq. (3.26) to gobble the leading kˆ factor, leaving F(k) = 1 + kˆ E e− jk·x = E + Ikˆ × E e− jk·x. (3.32)

It is also noteworthy that the directions kˆ, Eˆ , Hˆ form a right handed triple, which can be seen by computing their product

(kˆEˆ )Hˆ = (−Eˆ kˆ)(−IkˆEˆ ) = +IEˆ 2kˆ 2 (3.33) = I.

These vectors must all be mutually orthonormal for their product to be a pseudoscalar multiple. Should there be doubt, explicit dot products may be computed with ease using grade selection operations D E D E kˆ · Hˆ = kˆ(−IkÊˆ ) = − IEˆ = 0 D E D E (3.34) Eˆ · Hˆ = Eˆ (−IkÊˆ ) = − Ikˆ = 0, where the zeros follow by noting that IEˆ , Ikˆ are both bivectors. The conventional representation of the right handed triple relationship between the propagation direction and fields is stated as a cross product, not as a pseudoscalar relationship as in eq. (3.33). These are easily seen to be equivalent

kˆ = IHˆ Eˆ = I(Hˆ ∧ Eˆ ) (3.35) = I2(Hˆ × Eˆ ) = Eˆ × Hˆ .

3.5 statics.

3.5.1 Inverting the Maxwell statics equation.

Similar to electrostatics and magnetostatics, we can restrict attention to time invariant ﬁelds (∂tF = 0) and time invariant sources (∂t J = 0), but consider both electric and magnetic sources. In that case Maxwell’s equation is reduced to an invertible ﬁrst order gradient equation ∇F(x) = J(x), (3.36) 142 electromagnetism.

Theorem 3.4: Maxwell’s statics solution.

The solution to the Maxwell statics equation is given by

1 Z h(x − x0)J(x0)i F(x) = dV0 1,2 + F , 0 3 0 4π V kx − x k

where F0 is any function for which ∇F0 = 0. The explicit expansion in electric and magnetic ﬁelds and charge and current densities is given by ! 1 Z 1 1 E(x) = dV0 (x − x0)ρ(x0) + (x − x0) × M(x0) 0 3 4π V kx − x k ! 1 Z 1 1 H(x) = dV0 J(x0) × (x − x0) + (x − x0)ρ (x0) . 0 3 m 4π V kx − x k µ

We see that the solution incorporates both a Coulomb’s law contribution and a Biot-Savart law contribution, as well as their magnetic source analogues if applicable. To prove theorem 3.4, we utilize the Green’s function for the (ﬁrst order) gradient eq. (2.144), ﬁnding immediately

Z F(x) = dV0G(x, x0)∇0 J(x0) V *Z + = dV0G(x, x0)∇0 J(x0) (3.37) V 1,2 * + 1 Z (x − x0)J(x0) = dV0 . 0 3 4π V kx − x k 1,2

Here a no-op grade selection has been inserted to simplify subsequent manipulation2. We are also free to add any grade 1,2 solution of the homogeneous gradient equation, which provides the multivector form of the solution. To unpack the multivector result, let s = x − x0, and expand the grade 1,2 selection

hsJi1,2 = ηhs(cρ − J)i1,2 + hsI(cρm − M)i1,2 = ηcsρ − η(s ∧ J) + cIsρm − I(s ∧ M) (3.38) 1 = sρ + ηI(J × s) + scρ I + s × M, m

2 If this grade selection filter is omitted, it is possible to show that the scalar and pseudoscalar contributions to the (x − x0)J product are zero on the boundary of the Green’s integration volume. [16] 3.5 statics. 143 so the field is ! 1 Z 1 1 F(x) = dV0 sρ + s × M 4π kx − x0k3 V (3.39) 1 Z 1 + I dV0 (scρ + ηJ × s) . 0 3 m 4π V kx − x k Comparing this expansion to the field components F = E + ηIH, we complete the proof.

3.5.2 Enclosed charge.

In conventional electrostatics we obtain a relation between the normal electric field component and the enclosed charge by integrating the electric field divergence. The geometric algebra generalization of this relates the product of the normal and the electromagnetic field strength related to the enclosed multivector current

Theorem 3.5: Enclosed multivector current.

The enclosed multivector current in the volume is related to the surface integral of nˆ F over the boundary of the volume by Z Z dA nˆ F = dV J. ∂V V This is a multivector equation, carrying information for each grade in the multivector current. That grade selection yeilds

Z 1 Z dA nˆ · E = dV ρ ∂V V Z Z dA nˆ × H = dV J ∂V V Z Z dA nˆ × E = − dV M ∂V V Z 1 Z dA nˆ · H = dV ρm. ∂V µ V

To prove theorem 3.5 simply evaluate the volume integral of the gradient of the ﬁeld using theorem 2.11 Z Z dV∇F = dAnˆ F, (3.40) V ∂V 144 electromagnetism.

and note that Z Z dV∇F = dVJ. (3.41) V V This is a multivector relationship, containing a substantial amount of information, which can be extracted by expanding nˆ F

nˆ F = nˆ (E + IηH) = nˆ · E + I(nˆ × E) + Iη (nˆ · H + Inˆ × H) (3.42) = nˆ · E − η(nˆ × H) + I(nˆ × E) + Iη(nˆ · H).

Inserting this into theorem 3.5, and equating grades, we ﬁnd Z Z 1 dAnˆ · E = dV ρ ∂V V Z Z − dAη(nˆ × H) = − dVηJ ∂V V Z Z (3.43) I dA(nˆ × E) = −I dVM ∂V V Z Z I dAη(nˆ · H) = I dVcρm, ∂V V which completes the proof after cancelling common factors and some minor adjustments of the multiplicative constants. Of course eq. (3.43) could have obtained directly from Maxwell’s equations in their conventional form eq. (3.1). However, had we integrated the conventional Maxwell’s equations, it would not have been obvious that the crazy mix of ﬁelds, sources, dot R R and cross products in eq. (3.41) had a hidden structure as simple as ∂V dAnˆ F = V dVJ.

3.5.3 Enclosed current.

In this section we will present the generalization of Ampere’s law to line integrals of the total electromagnetic ﬁeld strength.

Theorem 3.6: Line integral of the ﬁeld.

The line integral of the electromagnetic ﬁeld strength is ! Z ∂F dx F = I dA nˆ J − , ∂A A ∂n

3.5 statics. 145

where ∂F/∂n = (nˆ · ∇) F. Expressed in terms of the conventional consistent ﬁelds and sources, this multivector relationship expands to four equations, one for each grade Z dx · E = dA nˆ · M ∂A A Z ! nˆρm ∂H dx × H = dA −nˆ × J + − ∂A A µ ∂n Z ! nˆρ ∂E dx × E = dA nˆ × M + − ∂A A ∂n Z dx · H = − dA nˆ · J. ∂A A

The last of the scalar equations in theorem 3.6 is Ampere’s law Z dx · H = nˆ · J = Ienc, (3.44) ∂A A

and the first is the dual of Ampere’s law for (fictitious) magnetic current density3. In eq. (3.44) the flux of the electric current density equals the enclosed current flowing through an open surface. This enclosed current equals the line integral of the magnetic field around the boundary of that surface. To prove theorem 3.6 we compute the surface integral of the current J = ∇F Z Z d2x J = d2x∇F. (3.45) A A

As we are working in R3 not R2, the gradient may not be replaced by the vector derivative in eq. (3.45). Instead we must split the gradient into its vector derivative component, the projection of the gradient onto the tangent plane of the integration surface, and its normal component ∇ = ∂ + nˆ(nˆ · ∇). (3.46)

The surface integral form eq. (2.89) of the fundamental theorem of geometric calculus may be applied to the vector derivative portion of the ﬁeld integral Z Z Z d2x∇F = d2x ∂F + d2x nˆ (nˆ · ∇) F, (3.47) A A A

3 Even without the ﬁctitious magnetic sources, neither the name nor applications of the two cross product line integrals with the normal derivatives are familiar to the author. 146 electromagnetism.

so Z dx F = d2x (J − nˆ (nˆ · ∇) F) ∂A ZA = dA (Inˆ J − (nˆ · ∇) IF) (3.48) A ! Z ∂F = dA Inˆ J − I , A ∂n

where the surface area bivector has been written in its dual form d2x = InˆdA in terms of a scalar area element, and the directional derivative has been written in scalar form with respect to a parameter n that represents the length along the normal direction. This proves the ﬁrst part of theorem 3.6. Observe that the dx F product has all possible grades

dx F = dx (E + IηH) = dx · E + Iηdx · H + dx ∧ E + Iηdx ∧ H (3.49) = dx · E − η(dx × H) + I(dx × E) + Iη(dx · H),

as does the Inˆ J product (in general)

ρ Inˆ J = Inˆ − ηJ + I (cρ − M) m ρ = nˆ I − ηnˆ IJ − nˆcρ + nMˆ (3.50) m ρ = nˆ · M + η(nˆ × J) − nˆcρ + I(nˆ × M) + nˆ I − ηI(nˆ · J). m On the other hand IF = IE − ηH has only grades 1,2, like F itself. This allows the line integrals to be split by grade selection into components with and without a normal derivative Z hdx Fi0,3 = dA hInˆ Ji0,3 ∂A A Z (3.51)

hdx Fi1,2 = dA (hInˆ Ji1,2 − (nˆ · ∇) IF) . ∂A A The ﬁrst of eq. (3.51) contains Ampere’s law and its dual as one multivector equation, which can be seen more readily by explicit expansion in the constituent ﬁelds and sources using eq. (3.49), eq. (3.50) Z (dx · E + Iη(dx · H)) = dA (nˆ · M − ηI(nˆ · J)) ∂A A Z (3.52) ! ρ ∂ (−η(dx × H) + I(dx × E)) = dA η(nˆ × J) − nˆcρm + I(nˆ × M) + nˆ I − (IE − ηH) . ∂A A ∂n

3.5 statics. 147

Further grade selection operations, and minor adjustments of the leading constants completes the proof. It is also worth pointing out that for pure magnetostatics problems where J = ηJ, F = IηH, that Ampere’s law can be written in a trivector form Z Z dx ∧ F = I dA nˆ · J = Iη dA nˆ · J. (3.53) ∂A A A This encodes the fact that the magnetic ﬁeld component of the total electromagnetic ﬁeld strength is most naturally expressed in geometric algebra as a bivector.

3.5.4 Example ﬁeld calculations.

Having seen a number of theoretical applications of the geometric algebra framework, let’s now see how some of our new tools can be used to calculate the fields for specific static electromagnetism charge and current configurations.

3.5.4.1 Line segment.

In this example the (electric) field is calculated at a point on the z-axis, due to a finite line charge density of λ along a segment [a, b] of the x-axis. The geometry of the problem is illustrated in fig. 3.1.

' x = re1ei x - x

' x = xe1 e1

Figure 3.1: Line charge density.

This is a fairly simple problem, and can be found in most introductory electromagnetic texts, usually set with the field observation point on the z-axis, and with a symmetric interval [−l/2, l/2], which has the side effect of killing off all but the x-axis component of the field. 148 electromagnetism.

For comparision purposes, this problem will be tackled ﬁrst using conventional algebra, and then using geometric algebra.

Conventional approach. The integral we wish to evaluate is

λ Z b (r cos θ − x)e + r sin θe E(x) = dx 1 3 . (3.54) 3/2 4π a r2 + x2 − 2rx cos θ This can be non-dimensionalized with a u = x/r change of variables, and yields an integral for the x component and the z component of the ﬁeld

λ Z b/r cos θ − u E = du x 3/2 4πr a/r (1 + u2 − 2u cos θ) (3.55) Z b/r λ sin θ 2 −3/2 Ey = du 1 + u − 2u cos θ . 4πr a/r There is a common integral in the x and y components of the ﬁeld. We can tidy this up a bit by writing

Z b/r −3/2 A = du 1 + u2 − 2u cos θ a/r Z b/r (3.56) −3/2 B = udu 1 + u2 − 2u cos θ , a/r and then put the pieces back together again for the total ﬁeld λ E = ((A cos θ − B)e + A sin θe ) . (3.57) 4πr 1 3 Some additional structure can be imposed by introducing a rotation matrix to express the ﬁeld observation point

x = rRθe1, (3.58)

where   cos θ 0 − sin θ   Rθ =  0 1 0  . (3.59)   sin θ 0 cos θ 

Writing 1 for the R3 identity matrix, the ﬁeld is λ E = (AR − B1) e . (3.60) 4πr θ 1 3.5 statics. 149

In retrospect we could have started using eq. (3.58) and obtained this result more directly. The A integral above results in both scaling and rotation of the ﬁeld, depending on the observation point and the limits of the integration. The B integral contributes only to the x-axis oriented component of the ﬁeld.

Using geometric algebra. Introducing a unit imaginary i = e13 for the rotation from the x-axis to the z-axis, the ﬁeld point observation point is

iθ x = re1e . (3.61)

0 The charge element point is x = xe1, so the diﬀerence can now be written with e1 factored to the left or to the right

0 iθ −iθ x − x = e1 re − x = re − x e1. (3.62)

These left and right factors can be used to convert the squared length of x − x0 into from a vector product into a product of conventional looking complex conjugates

02 −iθ iθ x − x = re − x e1e1 re − x (3.63) = re−iθ − x reiθ − x , so the squared length of the diﬀerence is

 − 02 2 2 − iθ −iθ x x = r + x rx e + e (3.64) = r2 + x2 − 2rx cos θ, and the total (electric) ﬁeld is

λ Z b re eiθ − xe F = dx 1 1 3/2 4π a 2 2 − r + x 2xr cos θ (3.65) λe Z b/r eiθ − u = 1 du . 3/2 4πr a/r 1 + u2 − 2u cos θ We have replaced the matrix representation that had nine components, four zeros, and a lot of redundancy with a simple multivector result. Moreover, the integral factor has the appearance of a conventional complex integral, and we can toss it as is into any numerical or symbol integration systems capable of complex number integrals for evaluation. The end result is a single vector valued inverse radial factor λe1/(4πr), multiplying by an integral that served to either scale or rotate-and-scale. 150 electromagnetism.

In particular, for θ = π/2, plugging this integral into Mathematica, we ﬁnd Z eiθ − u 1 + iu du = , (3.66) 3/2 p 1 + u2 − 2u cos θ 1 + u2 and for other angles θ , nπ/2 p Z eiθ − u (1 − ue−iθ) 1 + u2 − 2u cos θ du = . (3.67) 1 + u2 − 2u cos θ3/2 (1 + u2) sin(2θ) −iθ The numerator factors like e1(1 + iu) and e1(1 − ue ) compactly describe the direction of the vector ﬁeld at the observation point. Either of these can be expanded explicitly in sines and cosines if desired

e1(1 + iu) = e1 + ue3 −iθ (3.68) e1(1 − ue ) = e1(1 − u cos θ) + ue3 sin θ. Perhaps more interesting than the precise form of the solution is the fact that geometric algebra allows for the introduction of a “complex plane” for many problems that have only two degrees of freedom. When such a complex plane is introduced, existing Computer Algebra Systems (CAS), like Mathematica, can be utilized for the grunt work of the evaluation.

3.5.4.2 Inﬁnite line current.

Given a static line charge density and current density along the z-axis ρ(x) = λδ(x)δ(y) (3.69) J(x) = vρ(x) = vλe3δ(x)δ(y), the total multivector current is

J = η(cρ − J) = η(c − ve3)λδ(x)δ(y) (3.70) λ v = 1 − e δ(x)δ(y). c 3 We can find the field for this current using theorem 3.4. To do so, let the field observation point be x = x⊥ + ze3, so the total field is Z 0 λ h(x − x )(1 − (v/c)e3)i F(x) = dx0dy0dz0 1,2 δ(x0)δ(y0) 0 3 4π V kx − x k Z ∞ 0 λ h(x⊥ + (z − z )e3)(1 − (v/c)e3)i = dz0 1,2 3/2 (3.71) 4π −∞ 2 0 2 x⊥ + (z − z ) Z ∞ 0 Z ∞ 0 0 λ (x⊥ − (v/c)x⊥e ) dz λe (z − z )dz = 3 + 3 . 3/2 3/2 4π −∞ 2 0 2 4π −∞ 2 0 2 x⊥ + (z − z ) x⊥ + (z − z ) 3.5 statics. 151

2 The first integral is 2/x⊥, whereas the second is zero (odd function, over even interval). The bivector term of the grade selection above had a x⊥ ∧ e3 = x⊥e3 factor, which can be further reduced using cylindrical coordinates x = Rρˆ + ze3, since x⊥ = Rρˆ, which leaves λ v F(x) = ρˆ (1 − v/c) = E (1 − v/c) = E + I × E , (3.72) 2πR c where v = ve3. The vector component of this is the electric field, which is therefore directed radially, whereas the (dual) magnetic field ηIH is a set of oriented planes spanning the radial and z-axis directions. We can also see that there is a constant proportionality factor that relates the electric and magnetic field components, namely IηH = −Ev/c, (3.73) or H = v × D. (3.74)

Exercise 3.4 Linear magnetic density and currents.

Given magnetic charge density ρm = λmδ(x)δ(y), and current density M = ve3ρm = vρm, show that the ﬁeld is given by

λmc v F(x) = Iρˆ 1 − , 4πR c or with B = λmρˆ/(4πR),

F = B × v + cIB.

3.5.4.3 Inﬁnite planar current.

A variation on the above example puts a uniform charge density ρ(x) = σδ(z) in a plane, along iθ iθ with an associated current density J(x) = ve1e ρ(x), i = e12. Letting v = ve1e , the multivector current is J(x) = ση (c − v) δ(z), (3.75) so the ﬁeld oﬀ the plane is σ dz0dA0 F(x) = (x − x0)(1 − v/c) δ(z0). (3.76) 4π kx − x0k3 1,2 0 0 0 If xk = (x ∧ e3)$e3, and xk = (x ∧ e3)e3, are the components of the vectors x, x in the x-y 0 0 0 iθ0 plane, then integration over z and a change of variables xk − xk = r e1e yields 0 0 0 σ r dr dθ D 0 iθ0 E F(x) = ze3 − r e1e (1 − v/c) . (3.77) 4π (z2 + r02)3/2 1,2 " 152 electromagnetism.

0 The eiθ integrands are killed, so for z , 0, the ﬁeld is σz F(x) = he (1 − v/c)i . (3.78) 4π|z| 3 1,2

Since v ∈ span {e1, e2} the product e3v is a bivector and the grade selection can be dropped, leaving σ sgn(z) v F(x) = e 1 − . (3.79) 4π 3 c This ﬁeld toggles sign when crossing the plane, but is constant otherwise. The electric and magnetic ﬁeld components are once again related by eq. (3.74).

Exercise 3.5 Planar magnetic density and currents. iθ Given magnetic charge density ρm = σmδ(z), and current density M = vρm, v = ve1e , i = e12, show that the ﬁeld is given by σ c sgn(z) v F(x) = m i 1 − . 4π c

3.5.4.4 Arc line charge.

In this example we will examine the (electric) field due to a line charge density of λ along a circular arc segment φ0 ∈ [a, b], of radius r in the x-y plane. The field will be evaluated at the spherical coordinate point (R, θ, φ), as illustrated in fig. 3.2. Using the GA spherical parameterization of eq. (2.58), and eq. (2.59), the observation point now has the simple representation jθ x = Re3e , (3.80) and is the product of a polar directed vector with a complex exponential whose argument is the polar rotation angle. The bivector j is a function of the azimuthal angle φ, and encodes all the geometry of the rotation. To sum the contributions of the charge elements we need the distance between the charge element and the observation point. That vector difference is 0 jθ iφ0 x − x = Re3e − re1e . (3.81) Compare this to the tuple representation x − x0 = (R sin θ cos φ − r cos φ0, R sin θ sin φ − r cos φ0, cos θ), (3.82)

for which the prospect of working with is considerably less attractive. The squared length of eq. (3.81) is

0 2 2 2 jθ iφ0 (x − x ) = R + r − 2Rr e3e · e1e . (3.83) 3.5 statics. 153

Figure 3.2: Circular line charge. 154 electromagnetism.

The dot product of unit vectors in eq. (3.83) can be reduced using scalar grade selection

 jθ iφ0 D iφ iφ0 E e3e · e1e = e1 sin θe e1e D 0 E = sin θ e−iφeiφ (3.84) = sin θ cos(φ0 − φ),

so q 0 x − x = R2 + r2 − 2Rr sin θ cos(φ0 − φ). (3.85)

The electric ﬁeld is

0 1 Z b Re e jθ − re eiφ F = λrdφ0 3 1 . (3.86) 3/2 4π0 a R2 + r2 − 2Rr sin θ cos(φ0 − φ)

Non-dimensionalizing eq. (3.86) with u = r/R, a change of variables α = φ0 − φ, and noting iφ that iφˆ = e1e , the ﬁeld is

λr Z b−φ e e jθ − ue eiφeiα F = dα 3 1 2 3/2 4π0R a−φ 2 − 1 + u 2u sin θ cos α (3.87) Z b−φ λr rˆ + φˆuieiα = dα , 2 3/2 4π0R a−φ 1 + u2 − 2u sin θ cos α or    λr Z b−φ dα  F = r   ˆ  2 3/2  4π0R a−φ (1 + u2 − 2u sin θ cos α)   (3.88)  λrui Z b−φ eiαdα  + φˆ   .  2 3/2  4π0R a−φ (1 + u2 − 2u sin θ cos α)

Without CAS support for GA, this pair of integrals has to be evaluated separately. The first integral scales the radial component of the electric field. The second integral scales and rotates 0 φˆ within the azimuthal plane, producing an electric field component in a φˆ = φêiΦ direction.

3.5.4.5 Field of a ring current.

Let’s now compute the ﬁeld due to a static charge and current density on a ring of radius R as illustrated in ﬁg. 3.3. A static charge distribution on a ring at z = 0 has the form ρ(x) = λδ(z)δ(r − R). (3.89) 3.5 statics. 155

Figure 3.3: Field due to a circular distribution.

As always the current distribution is of the form J = vρ, and in this case the velocity is iφ azimuthal v = e2e , i = e12. The total multivector current is 1 v J = λδ(z)δ(r − R) 1 − . (3.90) c Let the point that we observe the ﬁeld, and the integration variables be

x = ze3 + rρˆ 0 0 0 0 (3.91) x = z e3 + r ρˆ . The ﬁeld is

D 0 E − 0 − 0 0 − v iφ λ (z z )e3 + rρˆ r ρˆ 1 c e2e F(x) = dz0r0dr0dφ0δ(z0)δ(r0 − R) 1,2 4π − 0 2 − 0 0 23/2 (z z ) + (rρˆ r ρˆ ) (3.92) D 0 E Z$ − 0 − v iφ λ ze3 + rρˆ Rρˆ 1 c e2e = Rdφ0 1,2 . 0 3/2 4π z2 + (rρˆ − Rρˆ )2

Without loss of generality, we can align the axes so that ρˆ = e1, and introduce dimensionless variables z˜ = z/R (3.93) r˜ = r/R, which gives

D 0 v 0 E Z 2π − iφ − iφ λ z˜e3 + r˜e1 e1e 1 c e2e F = dφ0 1,2 . (3.94) 2 iφ0 23/2 4πR 0 z˜ + (r˜e1 − e1e ) 156 electromagnetism.

In the denominator, the vector square expands as

0 0 0 − iφ 2 − −iφ 2 − iφ (r˜e1 e1e ) = (r˜ e )e1(r˜ e ) (3.95) = r˜2 + 1 − 2r˜ cos(φ0),

and the grade selection in the numerator is iφ0 v iφ0 iφ0 z˜e3 + r˜e1 − e1e 1 − e2e = z˜e3 + r˜e1 − e1e c 1,2 (3.96) v 0 − z˜e eiφ + ri˜ cos(φ0) + i . c 31 Any of the exponential integrals terms are of the form

Z 2π Z 2π 0 dφ0eiφ f (cos(φ0)) = dφ0 cos(φ0) f (cos(φ0)), (3.97) 0 0 since the i sin φ0 f (cos(φ0) contributions are odd functions around φ0 = π. For general z, r the integrals above require numeric evaluation or special functions. Let

Z 2π 1 A = dφ0 3/2 0 1 + z˜2 + r˜2 − 2r˜ cos(φ0) (3.98a) − 4r˜ 4E (r−1)2+z2 = ˜ ˜ p z˜2 + (r˜ − 1)2 z˜2 + (r˜ + 1)2

Z 2π cos(φ0) B = dφ0 3/2 0 1 + z˜2 + r˜2 − 2r˜ cos(φ0) (3.98b) 2 2 − 4r˜ − 2 2 − 4r˜ 2 z˜ + r˜ + 1 E (r−1)2+z2 z˜ + (r˜ + 1) K (r−1)2+z2 = ˜ ˜ ˜ ˜ , p r˜ z˜2 + (r˜ − 1)2 z˜2 + (r˜ + 1)2 where K(m), E(m) are complete elliptic integrals of the first and second kind respectively. As seen in fig. 3.4, these functions are similar, both tailing off quickly with z, ρ, with largest values the ring. iφ iφ Finally, restoring generality by making the transformation e1 → e1e = ρˆ, e2 → e2e = φˆ, the field is now fully determined λ vi v F = z˜e + r˜ρˆ − A − ρˆ + (z˜e ρˆ + ri˜ ) B . (3.99) 4πR 3 c c 3 The field directions are nicely parameterized as multivector expressions, with the relative weightings in different directions scaled by the position dependent integral coefficients of eq. (3.98). 3.5 statics. 157

(a) (b)

Figure 3.4: (a) A(z˜, ρ˜). (b) B(z˜, ρ˜).

The multivector field can be separated into its respective electric and magnetic components by inspection λ E = hFi = (zA˜ e + ρˆ(rA˜ − B)) 1 4πR 3 1 λv (3.100) H = h−IFi1 = −e3 (A + rB˜ ) − φˆzA˜ , η0 4πR which, as expected, shows that the static charge distribution ρ ∝ λ4 only contributes to the electric field, and the static current distribution J ∝ vλ only contributes to the magnetic field. See fig. 3.5, fig. 3.6 for plots of the electric and magnetic field directional variation near z˜ = 0, and fig. 3.7 for larger z where the azimuthal component of the field dominates.

Figure 3.5: Electric ﬁeld direction for circular charge density distribution near z = 0.

Exercise 3.6 Magnetic sources on a ring.

4 ∝: proportional to. 158 electromagnetism.

Figure 3.6: Magnetic ﬁeld direction for circular current density distribution near z = 0.

Figure 3.7: Magnetic ﬁeld for larger z. 3.5 statics. 159

iφ Given a constant (magnitude) multivector current on a ring J = Iλmδ(z)δ(r − R)(c − ve2e ), i = e12, show that the ﬁeld is

λmc v v F = zi˜ + r˜φˆe + e A + e φˆ + (z˜ρˆ − r˜e ) B . 4πR 3 c 3 3 c 3

3.5.4.6 Ampere’s law. Two current sources.

Let’s try using Ampere’s law as stated in theorem 3.6 two compute the field at a point in the blue region illustrated in fig. 3.8. This represents a pair of z-axis electric currents of magnitude I1, I2 flowing through the z = 0 points p1, p2 on the x-y plane.



I 1

e 1

Figure 3.8: Magnetic ﬁeld between two current sources.

Solving the system with superposition, let’s consider first one source flowing through p = (px, py, 0) with current J = e3Ieδ(x − px)δ(y − py), and evaluate the field due to this source at the point r. With only magnetic sources in the multivector current, Ampere’s law takes the form Z dxF = −I dAe3(−ηJ) = IηIe. (3.101) ∂A A The field F must be a bivector satisfying dx · F = 0. The circle is parameterized by

iφ r = p + Re1e , (3.102) so

iφ dx = Re2e dφ = Rφˆdφ. (3.103) 160 electromagnetism.

With the line element having only a φˆ component, F must be a bivector proportional to e3rˆ. Let iφ F = F0e31e , where F0 is a scalar, so that drF is a constant multiple of the unit pseudoscalar

Z 2π Z 2π iφ iφ drF = RF0 e2e dφe31e 0 0 Z 2π (3.104) −iφ iφ = RF0 e231e e dφ 0 = 2πIRF0,

1 F0 = IIe I2πR (3.105) I = e . 2πR The ﬁeld strength relative to the point p is

ηIe F = e3rˆ 2πR (3.106) ηIe = e rˆ. 2πR 3

Switching to an origin relative coordinate system, removing the z = 0 restriction for r and pk, and summing over both currents, the total ﬁeld at any point r strictly between the currents is

X ηIk 1 F = e3 2π e3 (e3 ∧ (r − pk)) k=1,2 (3.107) X ηI 1 = k . 2π e ∧ (r − p ) k=1,2 3 k The bivector nature of a ﬁeld with only electric current density sources is naturally represented by the wedge product e3 ∧ (r − pk) which is a vector product of e3 and the projection of r − pk onto the x-y plane.

3.6 dynamics.

3.6.1 Inverting Maxwell’s equation.

Maxwell’s equation (theorem 3.1) is invertable using the Green’s function for the spacetime gradient theorem 2.19. That solution is 3.6 dynamics. 161

Theorem 3.7: Jeﬁmenkos solution.

The solution of Maxwell’s equation is given by Z ! 1 rˆ 1 F(x, t) = F (x, t) + dV0 J(x0, t ) + (1 + rˆ) J˙ (x0, t ) , 0 4π r2 r cr r

where F0(x, t) is any specific solution of the homogeneous equation (∇ + (1/c)∂t) F0 = 0, time derivatives are denoted by overdots, and all times are evaluated at the retarded time tr = t − r/c. When expanded in terms of the electric and magnetic fields (ignoring magnetic sources), the non-homogeneous portion of this solution is known as Jefimenkos’ equations [8].

Z 0 0 ! ! 1 rˆ ρ(x , t ) ρ˙(x , t ) η E = dV0 r + r − J˙(x0, t ) 4π r r c cr r ! (3.108) 1 Z 1 1 H = dV0 J˙(x0, t ) + J(x0, t ) × rˆ, 4π cr r r2 r

The full solution is

Z 0 0 0 0 0 0 F(x, t) = F0(x, t) + dV dt G(x − x , t − t )J(x , t ) Z ! ! (3.109) 1 rˆ ∂ rˆ 1 ∂ = F (x, t) + dV0dt0 − + + δ(−r/c + t − t0) J(x0, t0) 0 4π r2 ∂r r cr ∂t where r = x − x0, r = krk and rˆ = r/r. With the help of eq. (C.18), the derivatives in the Green’s function eq. (3.109) can be evaluated, and the convolution reduces to Z ! ! 1 rˆ rˆ 1 d 1 d dt0G(x − x0, t − t0)J(x0, t0) = J(x0, t ) − − J(x0, t ) + J(x0, t ) . 4π r2 r r c dt r cr dt r r r tr=t−r/c (3.110)

There have been lots of opportunities to mess up with signs and factors of c, so let’s expand this out explicitly for a non-magnetic current source J = ρ/ − ηJ. Neglect the contribution of the homogeneous solution F0, and utilizing our freedom to insert a no-op grade 1,2 selection 162 electromagnetism.

operation, that removes any scalar and pseudoscalar terms that are necessarily killed over the full integration range, we ﬁnd

Z * !+ 1 rˆ ρ 1 ρ˙ F = dV0 − ηJ + (1 + r) − ηJ˙ 2 ˆ 4π r cr 1,2 Z ! 1 rˆ rˆ η 1 ρ˙ η = dV0 ρ − η ∧ J − J˙ + rˆ − rˆ ∧ J˙ (3.111) 4π r2 r2 cr cr cr Z  ˙  1 0  rˆ rˆρ˙ ηJ η η  = dV  ρ + − − I rˆ × J˙ − I rˆ × J . 4π r2 cr cr cr r2 

As F = E + IηH, the respective electric and magnetic ﬁelds by inspection. After re-inserting the space and time parameters that we suppressed temporarily, the proof is complete. The disadvantages of separating the ﬁeld and current components into their constituent components is also made painfully obvious by the complexity of the conventional statement of the solution compared to the equivalent multivector form.

3.7 energy and momentum.

3.7.1 Field energy and momentum density and the energy momentum tensor.

It is assumed here that the conventional definitions of the field energy and momentum density are known to the reader, as well as the conservation equations relating their space and time derivatives. For reference, the conventional definitions of those densities follow.

Deﬁnition 3.4: (Conventional) Energy and momentum density and Poynting vector.

The quantities E and P deﬁned as

1 E = E2 + µH2 2 1 Pc = E × H, c

are known respectively as the ﬁeld energy density and the momentum density. S = c2P = E × H is called the Poynting vector.

We will derive the conservation relationships that justify calling E, P the energy and momentum densities, and will also show that the Poynting vector represents the energy ﬂux through a surface per unit time. 3.7 energy and momentum. 163

In geometric algebra, it is arguably more natural to write the Poynting vector as a bivector- vector dot product such as 1 S = (IηH) · E, (3.112) η since this involves only components of the total electromagnetic ﬁeld strength F = E + IηH. However, we can do better, representing both E and S in terms of F directly. The key to doing so is making use of the fact that the energy and momentum densities are themselves components of a larger symmetric rank-2 energy momentum tensor, which can in turn be represented compactly in geometric algebra.

Deﬁnition 3.5: (Conventional) energy momentum and Maxwell stress tensors.

The rank-2 symmetric tensor Θµν, with components Θ00 = E2 + η2H2 2 1 Θ0i = (E × H) · e c i ! 1 Θi j = − E E + η2H H − δ E2 + η2H2 , i j i j 2 i j

is called the energy momentum tensor. The spatial index subset of this tensor is known as the Maxwell stress tensor, and is often represented in dyadic notation

 ↔ X a· T · b = aiTi jb j, i, j or ↔ X a· T≡ aiTi je j i, j

i j where Ti j = −Θ .

Here we use the usual convention of Greek indices such as µ, ν for ranging over both time (0) and spatial {1, 2, 3} indexes, and and Latin letters such as i, j for the “spatial” indexes {1, 2, 3}. The names and notation for the tensors vary considerably5.

5 Θµν in deﬁnition 3.5 is called the symmetric stress tensor by some authors [14], and the energy momentum tensor by others, and is sometimes written T µν ([17], [6]). The sign conventions and notation for the spatial components Θi j vary as well, but all authors appear to call this subset the Maxwell stress tensor. The Maxwell stress tensor may i j i j be written as σi j(= −Θ )[17], or as Ti j(= −Θ ) ([8], [14].) 164 electromagnetism.

In geometric algebra the energy momentum tensor, and the Maxwell stress tensor may be represented as linear grade 0,1 multivector valued functions of a grade 0,1 multivector.

Deﬁnition 3.6: Energy momentum and Maxwell stress tensors.

We deﬁne the energy momentum tensor as

1 T(a) = FaF†, 2 where a is a 0,1 multivector parameter. We introduce a shorthand notation for grade one selection with vector valued parameters

T(a) = hT(a)i1,

and call this the Maxwell stress tensor.

Theorem 3.8: Expansion of the energy momentum tensor.

P Given a scalar parameter α, and a vector parameter a = k akek, the energy momentum tensor of deﬁnition 3.6 is a grade 0,1 multivector, and may be expanded in terms of E, S and T(a) as ! S S T(α + a) = α E + − a · + T(a), c c

↔ i j where T(ei) · e j = −Θ , or T(a) = a· T. 3.7 energy and momentum. 165

Theorem 3.8 relates the geometric algebra definition of the energy momentum tensor to the quantities found in the conventional electromagnetism literature. Because T is a linear function of its parameter, we may prove this in parts, starting with α = 1, a = 0, which gives 1 T(1) = FF† 2 1 = (E + IηH)(E − IηH) 2 1 1 = E2 + η2H2 + Iη (HE − EH) 2 2 (3.113) 1 I = E2 + µH2 + H ∧ E 2 c 1 1 = E2 + µH2 + E × H 2 c S = E + . c An immediate take away from this expansion is that we may dispense with any requirement to refer to electric or magnetic field components in isolation and can express the energy and momentum densities (and Poynting) vector in terms of only the total electromagnetic field strength 1 D E E = FF† 2 1 D E Pc = FF† (3.114) 2 1 1 D E S = FF† . 2η 1 The power of this simple construction will be illustrated later when we compute the field energy and momentum densities for a number of Maxwell equation solutions in their geometric algebra form. An expansion of T(ek) is harder to do algebraically than eq. (3.113), but doing so will demonstrate that T(a) is a 0,1 grade multivector parameter for any grade 0,1 parameter6. Cheating a bit, here are the results of a brute force expansion of T(a) using a Mathematica GA computer algebra package

 η2 T(1) = E2 + E2 + E2 + H2 + H2 + H2 2 1 2 3 2 1 2 3 + e1η (E2H3 − E3H2) (3.115a) + e2η (E3H1 − E1H3)

+ e3η (E1H2 − E2H1)

6 Such an expansion is a worthwhile problem to develop GA manipulation skills. The reader is encouraged to try this independently ﬁrst, and to refer to appendixE for hints if required. 166 electromagnetism.

T(e1) = η (E3H2 − E2H3) 2 1 2 2 2 η 2 2 2 + e1 E − E − E + H − H − H 2 1 2 3 2 1 2 3 (3.115b) 2 + e2 E1E2 + η H1H2 2 + e3 E1E3 + η H1H3

T(e2) = η (E1H3 − E3H1) 2 + e1 E1E2 + η H1H2 1 η2 (3.115c) + e −E2 + E2 − E2 + −H2 + H2 − H2 2 2 1 2 3 2 1 2 3 2 + e3 E2E3 + η H2H3

T(e3) = η (E2H1 − E1H2) 2 + e1 E1E3 + η H1H3 2 (3.115d) + e2 E2E3 + η H2H3 1 η2 + e −E2 − E2 + E2 + −H2 − H2 + H2 2 3 1 2 3 2 1 2 3 Comparison to deﬁnition 3.5 shows that multivector energy momentum tensor is related to the conventional tensor representation by

0 00 hT(1)i = Θ0 = Θ i 0i hT(1)i1 · ei = Θ0 = Θ 0 i0 (3.116) hT(ei)i = Θi = −Θ j i j T(ei) · e j = Θi = −Θ = Ti j. 3.7 energy and momentum. 167

The only thing left to show is that how T(a) is equivalent to the dyadic notation found in ([8], [14]).

X T(a) = aiT(ei) i X = ai T(ei) · e j e j i, j (3.117) X = aiTi je j i, j ↔ = a· T .

The dyadic notation is really just a clumsy way of expressing the fact that T(a) is a linear vector valued function of a vector, which naturally has a matrix representation.

3.7.2 Poynting’s theorem (prerequisites.)

Poynting’s theorem is a set of conservation relationships between relating space and time change of energy density and momentum density, or more generally between related components of the energy momentum tensor. The most powerful way of stating Poynting’s theorem using geometric algebra requires a few new concepts, diﬀerential operator valued linear functions, and the adjoint.

Deﬁnition 3.7: Diﬀerential operator valued multivector functions.

Given a multivector valued linear functions of the form f (x) = AxB, where A, B, x are multivectors, and a linear operator D such as ∇, ∂t, or ∇ + (1/c)∂t, the operator valued linear function f (D) is deﬁned as

↔ ← → f (D) = A D B = (A D)B + A(D B),

↔ where D indicates that D is acting bidirectionally to the left and to the right.

Perhaps counter intuitively, using operator valued parameters for the energy momentum tensor T or the Maxwell stress tensor T will be particularly eﬀective to express the derivatives of the tensor. There are a few cases of interest, all related to evaluation of the tensor with a parameter value of the spacetime gradient. 168 electromagnetism.

Theorem 3.9: Energy momentum tensor operator parameters.

! 1 ∂T(1) 1 ∂ S T((1/c)∂ ) = = E + t c ∂t c ∂t c S hT(∇)i = −∇ · c X3 hT(∇)i1 = T(∇) = (∇ · T(ek)) ek. k=1

We will proceed to prove each of the results of theorem 3.9 in sequence, starting with the time partial, which is a scalar operator

 ↔ T(∂ ) = F ∂ F† t 2 t = (∂ F)F† + F(∂ F†) 2 t t (3.118) = ∂ FF† 2 t = ∂tT(1).

To evaluate the tensor at the gradient we have to take care of order. This is easiest in a scalar selection where we may cyclically permute any multivector factors

 ↔ hT(∇)i = F ∇ F† 2 D E = ∇F†F (3.119) 2 D E = ∇ F†F , 2 1 but

F†F = (E − IηH)(E + IηH) = E2 + η2H2 + Iη (EH − HE) (3.120) = E2 + η2H2 − 2ηE × H.

Plugging eq. (3.120) into eq. (3.119) proves the result. 3.7 energy and momentum. 169

Finally, we want to evaluate the Maxwell stress tensor of the gradient

X3 T(∇) = ek (T(∇)) · ek k=1 X3 = ek∂m (T(em) · ek) k,m=1 (3.121) X3 = ek∂m (T(ek) · em) k,m=1 X3 = ek (∇ · T(ek)) , k=1 as claimed. Will want to integrate T(∇) over a volume, which is essentially a divergence operation.

Theorem 3.10: Divergence integral for the Maxwell stress tensor.

Z Z dVT(∇) = dAT(nˆ). V ∂V

To prove theorem 3.10, we make use of the symmetric property of the Maxwell stress tensor

Z X Z dVT(∇) = dVek∇ · T(ek) V k V X Z = dAeknˆ · T(ek) k ∂V X Z = dAeknmT(ek) · em k,m ∂V (3.122) X Z = dAeknmT(em) · ek k,m ∂V X Z = dAekT(nˆ) · ek k ∂V Z = dAT(nˆ), ∂V as claimed. Finally, before stating Poynting’s theorem, we want to introduce the concept of an adjoint. 170 electromagnetism.

Deﬁnition 3.8: Adjoint.

The adjoint A(x) of a linear operator A(x) is deﬁned implicitly by the scalar selection D E yA(x) = hxA(y)i.

The adjoint of the energy momentum tensor is particularly easy to calculate.

Theorem 3.11: Adjoint of the energy momentum tensor.

The adjoint of the energy momentum tensor is T(x) = F† xF. 2

The adjoint T and T satisfy the following relationships D E T(1) = hT(1)i = E D E S T(1) = −hT(1)i = − 1 1 c D E S T(a) = −hT(a)i = a · c D E T(a) = hT(a)i = T(a). 1 1

Using the cyclic scalar selection permutation property hABCi = hCABi we form

D E hxT(y)i = xFyF† 2 D E (3.123) = yF† xF . 2 Referring back to deﬁnition 3.8 we see that the adjoint must have the stated form. Proving the grade selection relationships of eq. (3.123) has been left as an exercise for the reader. A brute force symbolic algebra proof using Mathematica is also available in appendixF. As in theorem 3.9, the adjoint may also be evaluated with diﬀerential operator parameters.

Theorem 3.12: Adjoint energy momentum tensor operator parameters. 3.7 energy and momentum. 171

D E 1 ∂T(1) 1 ∂E T((1/c)∂ ) = = t c ∂t c ∂t D E 1 ∂S T((1/c)∂ ) = − t 1 c2 ∂t D E S T(∇) = ∇ · c D E T(∇) = T(∇). 1

The proofs of theorem 3.12 are all fairly simple ! 1 ∂ 1 ∂ S T((1/c)∂ ) = F†F = E − . (3.124) t c 2 ∂t c ∂t c

D E D E T(∇) = 1T(∇) = h∇T(1)i (3.125) = ∇ · hT(1)i1 S = ∇ · . c

D E X D E T(∇) = ek ek · T(∇) 1 1 k X D E = ek ekT(∇) k X = ekh∇T(ek)i k (3.126) X = ek∇ · hT(ek)i1 k X = ek∇ · T(ek) k = T(∇).

3.7.3 Poynting theorem.

All the prerequisites for stating Poynting’s theorem are now ﬁnally complete.

Theorem 3.13: Poynting’s theorem (diﬀerential form.) 172 electromagnetism.

The adjoint energy momentum tensor of the spacetime gradient satisﬁes the following multivector equation T(∇ + (1/c)∂ ) = F† J + J†F . t 2

The multivector F† J + J†F can only have scalar and vector grades, since it equals its reverse. This equation can be put into a form that is more obviously a conservation law by stating it as a set of scalar grade identities

1 ∂ D E ∇ · hT(a)i + hT(a)i = a(F† J + J † F) , 1 c ∂t 2 or as a pair of scalar and vector grade conservation relationships

1 ∂E S 1 + ∇ · = − (E · J + H · M) c ∂t c c 1 ∂S − + T(∇) = ρE + E × M + ρ H + µJ × H. c2 ∂t m Conventionally, only the scalar grade relating the time rate of change of the energy density to the ﬂux of the Poynting vector, is called Poynting’s theorem. Here the more general multivector (adjoint) relationship is called Poynting’s theorem, which includes conservation laws relating for the ﬁeld energy and momentum densities and conservation laws relating the Poynting vector components and the Maxwell stress tensor.

The conservation relationship of theorem 3.13 follows from

! ! !† ! ! ↔ 1 ↔ 1 1 F† ∇ + ∂ F = ∇ + ∂ F F + F† ∇ + ∂ F c t c t c t (3.127) = J†F + F† J.

The scalar form of theorem 3.13 follows from D E 1 ∂ aT(∇ + (1/c)∂ ) = h(∇ + (1/c)∂ )T(a)i = ∇ · hT(a)i + hT(a)i. (3.128) t t 1 c ∂t We may use the scalar form of the theorem to extract the scalar grade, by setting a = 1, for which the right hand side can be reduced to a single term since scalars are reversion invariant

D E D E† D E F† J = F† J = J†F , (3.129) 3.7 energy and momentum. 173 so

1 ∂ S 1 ∂E ∇ · hT(1)i + hT(1)i = ∇ · + 1 c ∂t c c ∂t D E = F† J + J†F 2 D E = F† J (3.130)

= h(E − IηH)(η (cρ − J) + I (cρm − M))i = (−ηE · J − ηH · M) 1 1 = − E · J − H · M, c c which proves the claimed explicit expansion of the scalar grade selection of Poynting’s theorem. The left hand side of the vector grade selection follows by linearity using theorem 3.12 D E D E 1 ∂S T(∇ + (1/c)∂ ) = T(∇) + T((1/c)∂ ) = T(∇) − . (3.131) t 1 t 1 c2 ∂t The right hand side is a bit messier to simplify. Let’s do this in pieces by superposition, ﬁrst considering just electric sources

D E η e F† J + J†F = he ((E − IηH)(cρ − J) + (cρ − J)(E + IηH))i 2 k 2 k 1 = e · h(E − IηH)(cρ − J) + (cρ − J)(E + IηH)i 2c k 1 1 (3.132) = e · (cρE + IηH ∧ J) c k 1 = e · (cρE − ηH × J) c k = ek · (ρE + µJ × H) , and then magnetic sources

D E e F† J + J†F = he ((E − IηH)I(cρ − M) − I(cρ − M)(E + IηH))i 2 k 2 k m m = e · h(IE + ηH)(cρ − M) + (cρ − M)(−IE + ηH)i (3.133) 2 k m m 1 = ek · (ηcρmH − IE ∧ M) = ek · (ρmH + E × M) .

Jointly, eq. (3.131), eq. (3.132), eq. (3.133) complete the proof. The integral form of theorem 3.13 submits nicely to physical interpretation. 174 electromagnetism.

Theorem 3.14: Poynting’s theorem (integral form.)

∂ Z Z Z dV E = − dA nˆ · S − dV (J · E + M · H) ∂t V ∂V V Z Z ∂ Z Z dV (ρE + J × B) + dV (ρmH − M × E) = − dV P + dA T(nˆ). V V ∂t V ∂V (3.134)

Proof of theorem 3.14 requires only the divergence theorem, theorem 3.10, and definition 3.4. The scalar integral in theorem 3.14 relates the rate of change of total energy in a volume to the flux of the Poynting through the surface bounding the volume. If the energy in the volume increases(decreases), then in a current free region, there must be Poynting flux into(out-of) the volume. The direction of the Poynting vector is the direction that the energy is leaving the volume, but only the projection of the Poynting vector along the normal direction contributes to this energy loss. The right hand side of the vector integral in theorem 3.14 is a continuous representation of the Lorentz force (or dual Lorentz force for magnetic charges), the mechanical force on the charges in the volume. This can be seen by setting J = ρv (or M = ρmM) Z Z dV (ρE + J × B) = dVρ (E + v × B) V ZV (3.135) = dq (E + v × B) . V R As the field in the volume is carrying the (electromagnetic) momentum pem = V dVP, we can identify the sum of the Maxwell stress tensor normal component over the bounding integral as time rate of change of the mechanical and electromagnetic momentum Z dpmech dpem + = dAT(nˆ). (3.136) dt dt ∂V

3.7.4 Examples: Some static ﬁelds.

We’ve found solutions for a number of static charge and current distributions.

(a) For constant electric sources along the z-axis (eq. (3.72)) , with current J moving with velocity v = ve3, the ﬁeld had the form F = Eρˆ (1 − v/c). (b) For constant magnetic sources along the z-axis (exercise 3.4) , with current M moving with velocity v = ve3, the ﬁeld had the form F = ηHIρˆ (1 − v/c). 3.7 energy and momentum. 175

(c) For constant electric sources in the x-y plane (eq. (3.79)) , with current J moving with iθ velocity v = ve1e , i = e12, the ﬁeld had the form F = Ee3 (1 − v/c). (d) For constant magnetic sources in the x-y plane (exercise 3.5) , with current M moving with iθ velocity v = ve1e , i = e12, the ﬁeld had the form F = ηHi (1 − v/c).

In all cases the ﬁeld has the form F = A(1 − v/c), where A is either a vector or a bivector that anticommutes with the current velocity v, so the energy momentum tensor T(1) has the form

T(1) = A(1 − v/c)2A† 2 † = AA (1 + v/c)2 (3.137) 2 ! v2 v = AA† 1 + + 2 . 2 c c For the electric sources this is ! S v2 v E + = E2 1 + + 2 , (3.138) c 2 c c or ! v2 E = E2 1 + 2 c (3.139) S = E2v. For the magnetic sources this is ! S µ v2 v H + = H2 1 + + 2 , (3.140) c 2 c c or ! µ v2 H = H2 1 + 2 c (3.141) S = µH2v.

There are three terms in the multivector (1 − v/c)2 = 1 + (v/c)2 + 2v/c. For electric sources, the first scalar term is due to the charge distribution, and provides the electric field contribution to the energy density. The second scalar term is due to the current distribution, and provides the magnetic field contribution to the energy density. The final vector term, proportional to the current velocity contributes to the Poynting vector, showing that the field momentum travels along the direction of the current in these static configurations. Calculation of the T(ek) tensor components is generally more involved. Let’s do this calculation for each of the fields above in turn to illustrate. 176 electromagnetism.

(a): To calculate T(e3) we can reduce the following products

† 2 Fe3F = E ρˆ (1 − v/c) e3 (1 − v/c) ρˆ 2 2 = −E e3ρˆ (1 − v/c) ρˆ 2 2 2 = −E e3ρˆ 1 + v /c − 2v/c ρˆ (3.142) 2 2 2 2 = −E e3ρˆ 1 + v /c + 2v/c 2 2 2 = −E e3 1 + v /c + 2v/c .

Since S T(e ) = − · e + T(e ). (3.143) k c k k 2 This means that S · e3 = E v, as already found. The vector component of this tensor element is T(e ) = − E2e 1 + v2/c2 . (3.144) 3 2 3 This component of the stress tensor is aligned along the same axis as the velocity. Calculation of the other stress tensor components is easiest in cylindrical coordinates. Along the radial direction ρˆ (1 − v/c) ρˆ (1 − v/c) ρˆ = ρˆ 2 (1 + v/c)(1 − v/c) ρˆ (3.145) = 1 − v2/c2 ρˆ,

and along the azimuthal direction

ρˆ (1 − v/c) θˆ (1 − v/c) ρˆ = ρˆθˆ (1 + v/c)(1 − v/c) ρˆ = −θˆρˆ 2 1 − v2/c2 (3.146) = −θˆ 1 − v2/c2 .

Since T(a) is a linear operator for any vector parameters a, it cannot have any grade zero component along any directions e · e3 = 0. No grade zero component of T(e1), T(e2) implies that the Poynting vector is zero along the e1 and e2 directions respectively, as we saw above in eq. (3.139). In summary T(ρˆ) = E2 1 − v2/c2 ρˆ 2 T(θˆ) = − E2 1 − v2/c2 θˆ (3.147) 2 T(e ) = − E2 1 + v2/c2 e . 3 2 3 3.7 energy and momentum. 177

For this ﬁeld that T(ρˆ) is entirely radial, whereas T(θˆ) is entirely azimuthal. In terms of an arbitrary vector in cylindrical coordinates

a = aρρˆ + aθθˆ + aze3, (3.148) the grade one component of the tensor is T(a) = E2 1 − v2/c2 a ρˆ − a θˆ − E2 1 + v2/c2 a e . (3.149) 2 ρ θ 2 z 3

(b): For F = ηHIρˆ (1 − v/c), and v = ve3 we have

† 2 2 FaF = η H Iρˆ (1 − v/c) a (1 − v/c) ρˆ(−I) (3.150) = η2H2ρˆ (1 − v/c) a (1 − v/c) ρˆ.

We can write the tensor components immediately, since eq. (3.150) has exactly the same structure as the tensor components computed in part (a) above. That is µ µ T(a) = H2 1 − v2/c2 a ρˆ − a θˆ − H2 1 + v2/c2 a e . (3.151) 2 ρ θ 2 z 3

(c): For F = Ee3 (1 − v/c), and v = vρˆ, we have

† 2 FaF = E e3 (1 − (v/c)ρˆ) a (1 − (v/c)ρˆ) e3, (3.152) so we need the following grade selections

D 2 E e (1 − (v/c)ρˆ) ρˆ (1 − (v/c)ρˆ) e = e ρˆ (1 − (v/c)ρˆ) e 3 3 1 3 3 1 D E = e ρˆ 1 + (v2/c2) − 2(v/c)ρˆ e 3 3 1 2 2 = 1 + (v /c ) e3ρˆe3 = − 1 + (v2/c2) ρˆ D E D E e (1 − (v/c)ρˆ) θˆ (1 − (v/c)ρˆ) e = e θˆ (1 + (v/c)ρˆ)(1 − (v/c)ρˆ) e (3.153) 3 3 1 3 3 1 D E = e θˆ 1 − (v2/c2) e 3 3 1 = − 1 − (v2/c2) θˆ

e3 (1 − (v/c)ρˆ) e3 (1 − (v/c)ρˆ) e3 1 = (1 + (v/c)ρˆ)(1 − (v/c)ρˆ) e3 1 2 2 = 1 − (v /c ) e3.

So the Maxwell stress tensor components of interest are T(a) = − E2 1 + (v2/c2) a ρˆ + E2 1 − (v2/c2) a e − a θˆ . (3.154) 2 ρ 2 z 3 θ 178 electromagnetism.

(d): For F = ηHi (1 − v/c) , i = e12, and v = vρˆ, we can use a duality transformation for the unit bivector i

F = ηHIe3 (1 − v/c) , (3.155)

so † 2 2 FaF = η H e3 (1 − v/c) a (1 − v/c) e3. (3.156)

Equation (3.156) has the structure found in part (c) above, so µ µ T(a) = − H2 1 + (v2/c2) a ρˆ + H2 1 − (v2/c2) a e − a θˆ . (3.157) 2 ρ 2 z 3 θ

3.7.5 Complex energy and power.

Theorem 3.15: Complex power representation.

Given a time domain representation of a phasor based ﬁeld F = F(ω) F(t) = Re Fe jωt ,

the energy momentum tensor multivector T(1) has the representation

S T(1) = E + = Re F∗F† + FF†e2 jωt . c 4 With the usual deﬁnition of the complex Poynting vector

1 1 S = E × H∗ = (IH∗) · E, 2 2 the energy and momentum components of T(1), for real µ, are

1 1 E = |E|2 + µ|H|2 + Re E2 + µH2 e2 jωt 4 4 1 S = Re S + Re (E × H) e2 jωt . 2

To prove theorem 3.15 we start by expanding the real part operation explicitly

 F(t) = Re Fe jωt 1 (3.158) = Fe jωt + F∗e− jωt . 2 3.7 energy and momentum. 179

The energy momentum multivector for the ﬁeld is therefore

1 F(t)F(t)† = Fe jωt + F∗e− jωt F†e jωt + F∗† e− jωt 2 8 (3.159) ∗ ∗ = FF†e2 jωt + FF†e2 jωt + F∗F† + F∗F† , 8 so we have

S 1 E + = F(t)F(t)† c 2 (3.160) = Re F∗F† + FF†e2 jωt , 4 which proves the ﬁrst part of the theorem. Next, we’d like to expand T(1)

1 1 F∗F† = E∗ + IηH∗ (E − IηH) 4 4 1 = E∗E + η2H∗H + Iη H∗E − E∗H (3.161) 4 1 I = |E|2 + µ|H|2 + H∗E − E∗H . 4 c The scalar terms are already real, but the real part of the vector term is

I I Re H∗E − E∗H = H∗E − E∗H + HE∗ − EH∗ 4c 8c I = 2H∗ ∧ E + 2H ∧ E∗ 8c (3.162) 1 = E × H∗ + E∗ × H 4c 1 = Re E × H∗ . 2c The FF† factor of e2 jωt above was expanded in eq. (3.113), so the energy momentum multivector is S 1 1 E + = |E|2 + µ|H|2 + Re (E × H∗) c 4 2c ! ! (3.163) 1 1 + Re E2 + µH2 + E × H e2 jωt . 4 2c

Expressing eq. (3.163) in terms of the complex Poynting vector S, completes the proof. 180 electromagnetism.

Observe that averaging over one period T kills any sinusoidal contributions, so the steady state energy and Poynting vectors are just

1 Z τ+T 1 E(t)dt = |E|2 + µ|H|2 T 4 τ (3.164) 1 Z τ+T S(t)dt = Re S. T τ

3.8 lorentz force.

3.8.1 Statement.

We now wish to express the Lorentz force equation eq. (3.5a) in its geometric algebra form. A few deﬁnitions are helpful.

Deﬁnition 3.9: Energy momentum multivector.

For a particle with energy E and momentum p, we deﬁne the energy momentum multivector as

T = E + cp.

Deﬁnition 3.10: Multivector charge.

We may deﬁne a multivector charge that includes both the magnitude and velocity (relative to the speed of light) of the charged particle. Z Q = JdV, V

where J = ρeve, M = ρmvm. For electric charges this is

Q = qe (1 + ve/c) ,

and for magnetic charges

Q = Iqm (1 + vm/c) , R R where qe = V ρedV, qm = V ρmdV. 3.8 lorentz force. 181

With a multivector charge deﬁned, the Lorentz force equation can be stated in terms of the total electromagnetic ﬁeld strength

Theorem 3.16: Lorentz force and power.

The respective power and force experienced by particles with electric (and/or magnetic) charges is described by deﬁnition 3.10 is

1 dT D E 1 = FQ† = F†Q + FQ† . c dt 0,1 2

where hdT/dti = dE/dt is the power and hdT/dti1 = cdp/dt is the force on the particle, and Q† is the electric or magnetic charge/velocity multivector of deﬁnition 3.10. The conventional representation of the Lorentz force/power equations

D E dp FQ† = = q (E + v × B) 1 dt D E dE c FQ† = = qE · v. dt may be recovered by grade selection operations. For magnetic particles, such a grade selection gives ! D E dp 1 FQ† = = q cB − v × E 1 dt m c m D E dE 1 v c FQ† = = q B · m . dt η m c

To prove theorem 3.16, we can expand the multivector product Fq (1 + v/c) into its constituent grades

 v v qF 1 + = q (E + IcB) 1 + c c q = qE + qIBv + Ev + qcIB (3.165) c ! q 1 = E · v + q (E + v × B) + q cIB + E ∧ v + q(IB) ∧ v. c c 182 electromagnetism.

We see the (c-scaled) particle power relationship eq. (3.5b) in the grade zero component and the Lorentz force eq. (3.5b) in the grade 1 component. A substitution q → −Iqm, v → vm, and subsequent grade 0,1 selection gives

! vm 1 −IqmF 1 + = −Iqm cIB + E ∧ vm − IqmIB · vm c 0,1 c ! (3.166) 1 = q cB − v × E + q B · v . m c m m m

The grade one component of this multivector has the required form for the dual Lorentz force equation from theorem 3.14. Scaling the grade zero component by c completes the proof.

3.8.2 Constant magnetic ﬁeld.

The Lorentz force equation that determines the dynamics of a charged particle in an external field F has been restated as a multivector differential equation, but how to solve such an equation is probably not obvious. Given a constant external magnetic field bivector F = IcB, the Lorentz force equation is reduced to dv v m = qF · , (3.167) dt c or qF Ω = − mc (3.168) dv = v · Ω, dt where Ω is a bivector containing all the constant factors. This can be solved by introducing a multivector integration factor R and its reverse R† on the left and right respectively

dv R R† = Rv · ΩR† dt 1 = R (vΩ − Ωv) R† (3.169) 2 1 1 = RvΩR† − RΩvR†, 2 2 or dv 1 1 0 = R R† + RΩvR† − RvΩR†. (3.170) dt 2 2 3.8 lorentz force. 183

Let R˙ = RΩ/2. (3.171)

Since Ω is a bivector R˙ † = −ΩR†/2, so by chain rule d 0 = RvR† . (3.172) dt The integrating factor has solution

R = eΩt/2, (3.173) a “complex exponential”, so the solution of eq. (3.167) is

v(t) = e−Ωt/2v(0)eΩt/2. (3.174)

The velocity of the charged particle traces out a helical path. Any component of the initial velocity v(0)⊥ perpendicular to the Ω plane is untouched by this rotation operation, whereas components of the initial velocity v(0)k that lie in the Ω plane will trace out a circular path. If Ωˆ is the unit bivector for this plane, that velocity is

 −1 v(0)k = v(0) · Ωˆ Ωˆ = (v(0) ∧ Bˆ ) · Bˆ −1 v(0)⊥ = v(0) ∧ Ωˆ Ωˆ = (v(0) · Bˆ )Bˆ (3.175) Ωt v(t) = v(0)ke + v(0)⊥

= v(0)k cos(qBt/m) + v(0)k × Bˆ sin(qBt/m) + v(0)⊥, where B = BBˆ . A multivector integration factor method for solving the Lorentz force equation in constant external electric and magnetic ﬁelds can be found in [9]. Other examples, solved using a relativistic formulation of GA, can be found in [6], [11], and [12].

3.8.2.1 Problems.

Exercise 3.7 Constant magnetic ﬁeld.

−1 −1 Ωt In eq. (3.175), each of v(0) · Ωˆ Ωˆ , v(0) ∧ Ωˆ Ωˆ , and v(0)ke + v(0)⊥, was expanded by setting Ωˆ = IBˆ . Perform those calculations. 184 electromagnetism.

3.9 polarization.

3.9.1 Phasor representation.

In a discussion of polarization, it is convenient to align the propagation direction along a ﬁxed direction, usually the z-axis. Setting kˆ = e3, βz = k · x in a plane wave representation from theorem 3.3 the ﬁeld is − jβz F(x, ω) = (1 + e3)Ee (3.176) F(x, t) = Re F(x, ω)e jωt ,

where E · e3 = 0 , (i.e. E is an electric ﬁeld, and not just a free parameter). Here the imaginary j has no intrinsic geometrical interpretation, E = Er + jEi is allowed to have complex values, and all components of E is perpendicular to the propagation direction (Er · e3 = Ei · e3 = 0). Stated explicitly, this means that the electric ﬁeld phasor may have real or complex components in either of the transverse plane basis directions, as in

E = (α1 + jβ1) e1 + (α2 + jβ2) e2. (3.177) The total time domain ﬁeld for this general phasor ﬁeld is easily found to be

F(x, t) = (1 + e3) ((α1e1 + α2e2) cos (ωt − βz) − (β1e1 + β2e2) sin (ωt − βz)) . (3.178)

Diﬀerent combinations of α1, α2, β1, β2 lead to linear, circular, or elliptically polarized plane wave states to be discussed shortly. Before doing so, we want to ﬁnd natural multivector representations of eq. (3.178). Such representations are possible using either the pseudoscalar for the 3 transverse plane e12, or the R pseudoscalar I.

3.9.2 Transverse plane pseudoscalar.

3.9.2.1 Statement.

In this section the pseudoscalar of the transverse plane, written i = e12, is used as an imaginary. Deﬁnition 3.11: Phase angle.

Deﬁne the total phase as

φ(z, t) = ωt − βz.

We seek a representation of the ﬁeld utilizing complex exponentials of the phase, instead of signs and cosines. It will be helpful to deﬁne the coordinates of the Jones vector to state that representation. 3.9 polarization. 185

Deﬁnition 3.12: Jones vectors.

The coordinates of the Jones vector, conventionally deﬁned as a tuple of complex values (c1, c2), are

c1 = α1 + iβ1

c2 = α2 + iβ2.

In this deﬁnition we have used i = e12, the pseudoscalar of the transverse plane, as the imaginary.

We will not use the Jones vector as a tuple, but will use c1, c2 as stated above. Theorem 3.17: Circular polarization coeﬃcients.

The time domain representation of the ﬁeld in eq. (3.178) can be stated in terms of the total phase as

 iφ −iφ F = (1 + e3) e1 αRe + αLe ,

where 1 α = (c + ic ) R 2 1 2 1 α = (c − ic )† , L 2 1 2

where c1, c2 are the 0,2 grade multivector representation of the Jones vector coordinates from deﬁnition 3.12.

To prove theorem 3.17, we have only to factor e1 out of eq. (3.178) and then substitute complex exponentials for the sine and cosine

(α1e1 + α2e2) cos (φ) − (β1e1 + β2e2) sin (φ)

= e1 ((α1 + α2i) cos (φ) − (β1 + β2i) sin (φ)) e = 1 (α + α i) eiφ + e−iφ + (β + β i) i eiφ − e−iφ 2 1 2 1 2 (3.179) e = 1 (α + iβ + i(α + iβ )) eiφ + (α + iβ )† + i(α + iβ )† e−iφ 2 1 1 2 2 1 1 2 2 e = 1 (c + ic ) eiφ + (c − ic )† e−iφ , 2 1 2 1 2 which completes the proof. 186 electromagnetism.

3.9.2.2 Linear polarization.

Linear polarization is described by

1 i(ψ+θ) αR = kEk e 2 (3.180) 1 α = kEk ei(ψ−θ), L 2 so the ﬁeld is iψ F = (1 + e3) kEk e1e cos(ωt − βz + θ). (3.181)

Here θ is an arbitrary initial phase. The electric field E traces out all the points along the line iψ spanning the points between ±e1e kEk, whereas the magnetic field H traces out all the points iψ along ±e2e kEk /η as illustrated (with η = 1) in fig. 3.9.

i ψ e1E e

E i ψ e e2 e 2 η ψ e1

E i ψ -e2 e η

i ψ -e1E e

Figure 3.9: Linear polarization.

3.9.2.3 Circular polarization.

A ﬁeld for which the change in phase results in the electric ﬁeld tracing out a (clockwise,counterclockwise) circle

ER = kEk (e1 cos φ + e2 sin φ) = kEk e1 exp (e12φ) (3.182) EL = kEk (e1 cos φ − e2 sin φ) = kEk e1 exp (−e12φ) ,

is referred to as having (right,left) circular polarization, so the choice αR = kEk , αL = 0 results in a right polarized wave

i(ωt−kz) F = (1 + e3) kEk e1e , (3.183) 3.9 polarization. 187

and αL = kEk , αR = 0 results in a left polarized wave −i(ωt−kz) F = (1 + e3) kEk e1e , (3.184)

There are diﬀerent conventions for the polarization orientation, and here the IEEE antenna convention discussed in [2] are used.

3.9.2.4 Elliptical parameterization.

An elliptical polarized electric ﬁeld can be parameterized as

E = Eae1 cos φ + Ebe2 sin φ, (3.185) which corresponds to circular polarization coeﬃcients with values 1 αR = (Ea − Eb) 2 (3.186) 1 α = (E + E ) . L 2 a b Therefore an elliptically polarized ﬁeld can be represented as 1 F = (1 + e )e (E + E )eiφ + (E − E )e−iφ . (3.187) 2 3 1 a b a b An interesting variation of the elliptical polarization uses a hyperbolic parameterization. If a, b are the semi-major/minor axes of the ellipse (i.e. a > b), and a = ae eiψ is the vectoral 1 p 2 representation of the semi-major axis (not necessarily placed along e1), and e = 1 − (b/a) is the eccentricity of the ellipse, then it can be shown ([9]) that an elliptic parameterization can be written in the compact form r(φ) = ea cosh(tanh−1(b/a) + iφ). (3.188)

When the bivector imaginary i = e12 is used then this parameterization is real and has only vector grades, so the electromagnetic ﬁeld for a general elliptic wave has the form

iψ F = eEa (1 + e3) e1e cosh (m + iφ) −1 m = tanh (Eb/Ea) (3.189) q 2 e = 1 − (Eb/Ea) , where Ea(Eb) are the magnitudes of the electric field components lying along the semi-major(minor) axes, and the propagation direction e3 is normal to both the major and minor axis directions. An elliptic electric field polarization is illustrated in fig. 3.10, where the vectors representing the iψ iψ major and minor axes are Ea = Eae1e , Eb = Ebe1e . Observe that setting Eb = 0 results in the linearly polarized field of eq. (3.181). 188 electromagnetism.

Eb ψ e1

Figure 3.10: Electric ﬁeld with elliptical polarization.

3.9.2.5 Energy and momentum.

Each polarization considered above (linear, circular, elliptical) have the same general form

iψ F = (1 + e3) e1e f (φ), (3.190)

where f (φ) is a complex valued function (i.e. grade 0,2). The structure of eq. (3.190) could be more general than considered so far. For example, a Gaussian modulation could be added into 2 the mix with f (φ) = eiφ−(φ/σ) /2. Independent of the form of f , we may compute the energy, momentum and Maxwell stress tensor for the plane wave given by eq. (3.190).

Theorem 3.18: Energy momentum tensor components for a plane wave.

The energy momentum tensor components for the plane wave given by eq. (3.190) are ! S T(1) = −T(e ) = (1 + e ) f f † = E + 3 3 c

T(e1) = T(e2) = 0.

Only the propagation direction of a plane wave, regardless of its polarization (or even whether or not there are Gaussian or other damping factors), carries any energy or momentum, and only the propagation direction component of the Maxwell stress tensor T(a) is non-zero. To prove theorem 3.18, we may compute T(a) separately for each of a = 1, e1, e2, e3. Key to all of these computations is the fact that e3 commutes with scalars and i, and e1, e2 both 3.9 polarization. 189

    e1 e1 anticommute with i, and more generally   (a + ib) = (a − ib)  . For T(1) we need the     e2 e2 product of the ﬁeld and its reverse

† ¨ïψ † −ïψ¨ FF = (1 + e3)ë1e f f ë e1 (1 + e3)

scalar (3.191) 2 † = (1 + e3) f f † = 2 (1 + e3) f f ,

† so T(1) = (1 + e3) f f . For T(e3) we have

† iψ † −iψ Fe3F = (1 + e3) e1e f e3 f e e1 (1 + e3) iψ † −iψ = − (1 + e3) e3e1e f f e e1 (1 + e3) (3.192) iψ † −iψ = − (1 + e3) e1e f f e e1 (1 + e3) † = −2 (1 + e3) f f , so T(e3) = −T(1). For T(e1), we have

† iψ † −iψ Fe1F = (1 + e3) e1e f e1 f e e1 (1 + e3) iψ 2 iψ 2 = (1 + e3) e1e f e e1 (1 + e3) 2 2iψ = (1 + e3) e1 f e (1 + e3) 2 2iψ (3.193) = (1 + e3) e1 (1 + e3) f e 2 2iψ = (1 + e3)(1 − e3) e1 f e 2 2 2iψ = 1 − e3 e1 f e = 0.

† Clearly Fe2F = 0 as well, so T(e1) = T(e2) = 0, completing the proof. Using theorem 3.18 the energy momentum vector for the linearly polarized wave of eq. (3.181) is T(1) = (1 + e ) kEk2 cos2(φ + θ), (3.194) 2 3 and for the circularly polarized wave of eq. (3.183), or eq. (3.184) is T(1) = (1 + e ) kEk2 . (3.195) 2 3 A circularly polarized wave carries maximum energy and momentum, whereas the energy and momentum of a linearly polarized wave oscillates with the phase angle. 190 electromagnetism.

For the elliptically polarized wave of eq. (3.189) we have f (φ) = eEa cosh (m + iφ). The absolute value of f is

† 2 2 † f f = e Ea cosh (m + iφ)(cosh (m + iφ)) 2 2 = e Ea (cosh(2m) + cos(2φ))     (3.196)  E2  E2   = e2E2  b + 2 1 − b  cos2 φ a  2  2   Ea Ea The simpliﬁcation above made use of the identity (1 − (b/a)2) cosh(2 atanh(b/a)) = 1 + (b/a)2. The energy momentum for an elliptically polarized wave is therefore      E2  E2   T(1) = (1 + e ) e2E2  b + 2 1 − b  cos2 φ . (3.197) 3 a  2  2   2 Ea Ea As expected, the phase dependent portion of the energy momentum tensor vanishes as the wave function approaches circular polarization.

3.9.3 Pseudoscalar imaginary.

In this section we use the R3 pseudoscalar as an imaginary. As before, we seek a representation of the field utilizing complex exponentials of the phase, instead of signs and cosines, and as before the we wish to define Jones vector coordinates as a go-between. Definition 3.13: Jones vectors.

The coordinates of the Jones vector, conventionally deﬁned as a tuple of complex values (c1, c2), are

c1 = α1 + Iβ1

c2 = α2 + Iβ2.

In this deﬁnition we have used the R3 pseudoscalar I as the imaginary.

We will not use the Jones vector as a tuple, but will use c1, c2 as stated above. Theorem 3.19: Circular polarization coeﬃcients.

The time domain representation of the ﬁeld in eq. (3.178) can be stated in terms of the total phase as

 −Iφ Iφ F = (1 + e3) e1 αRe + αLe , 3.9 polarization. 191

where 1 α = (c + Ic )† R 2 1 2 1 α = (c − Ic ) , L 2 1 2

where c1, c2 are the 0,2 grade multivector representation of the Jones vector coordinates from definition 3.13. Notice that the signs of the exponentials have flipped for the left and right handed circular polarizations. It may not obvious that the electric and magnetic fields in this representation have the desired transverse properties. To see why that is still the case, and to understand the conjugation in the complex exponentials, consider the right circular polarization case with αR = kEk , αL = 0

−Iφ F = (1 + e3) e1 kEk e = (1 + e3) kEk (e1 cos φ − e23 sin φ) (3.198) = (1 + e3) kEk (e1 cos φ + e32 sin φ) , but since (1 + e3) e3 = 1 + e3, we have

F = (1 + e3) kEk (e1 cos φ + e2 sin φ) , (3.199) which has the claimed right circular polarization. To prove theorem 3.19 itself, the sine and cosine in eq. (3.178) can be expanded in complex exponentials

2 (α1e1 + α2e2) cos φ − 2 (β1e1 + β2e2) sin φ Iφ −Iφ Iφ −Iφ = (α1e1 + α2e2) e + e + (β1e1 + β2e2) I e − e (3.200) Iφ −Iφ Iφ −Iφ = (α1e1 − Iα2(Ie2)) e + e + (β1e1 − Iβ2(Ie2)) I e − e .

Since the leading 1 + e3 gobbles any e3 factors, its action on the dual of e2 is

(1 + e3) Ie2 = (1 + e3) e31 (3.201) = (1 + e3) e1.

This allows us to unconditionally factor out e1 from eq. (3.200), so the ﬁeld is 1 F = (1 + e ) e (α − Iα ) eIφ + e−Iφ + (β − Iβ ) I eIφ − e−Iφ 2 3 1 1 2 1 2 1 = (1 + e ) e (α + Iβ − I (α + Iβ )) eIφ + (α − Iβ − I (α − Iβ )) e−Iφ 2 3 1 1 1 2 2 1 1 2 2 (3.202) 1 = (1 + e ) e (c − Ic ) eIφ + c† − Ic† e−Iφ 2 3 1 1 2 1 2 −Iφ −Iφ = (1 + e3) e1 αRe + αLe , 192 electromagnetism.

which completes the proof. Observe that there are some advantages to the pseudoscalar plane wave form, especially for computing energy momentum tensor components since I commutes with all grades. For example, we can see practically by inspection that

S T(1) = E + = (1 + e ) |α |2 + |α |2 , (3.203) v 3 R L

where the absolute value is computed using the reverse as the conjugation operation |z|2 = zz†.

3.10 transverse fields in a waveguide.

We now wish to consider more general solutions to the source free Maxwell’s equation than the plane wave solutions derived in section 3.4. One way of tackling this problem is to assume the solution exists, but ask how the ﬁeld components that lie strictly along the propagation direction are related to the transverse components of the ﬁeld. Without loss of generality, it can be assumed that the propagation direction is along the z-axis.

Theorem 3.20: Transverse and propagation ﬁeld components.

If e3 is the propagation direction, the components of a ﬁeld F in the propagation direction and in the transverse plane are respectively

1 F = (F + e Fe ) z 2 3 3 1 F = (F − e Fe ) , t 2 3 3

where F = Fz + Ft.

To determine the components of the field that lie in the propagation direction and transverse planes, we state the field in the propagation direction, building it from the electric and magnetic field projections along the z-axis

Fz = (E · e3) e3 + Iη (H · e3) e3 1 1 = (Ee + e E) e + Iη (He + e H) e 2 3 3 3 2 3 3 3 1 1 (3.204) = (E + e Ee ) + Iη (H + e He ) 2 3 3 2 3 3 1 = (F + e Fe ) . 2 3 3 3.10 transverse fields in a waveguide. 193

The diﬀerence F − Fz is the transverse component

Ft = F − Fz 1 = F − (F + e Fe ) 2 3 3 (3.205) 1 = (F − e Fe ) , 2 3 3 as claimed. We wish to split the gradient into transverse and propagation direction components.

Deﬁnition 3.14: Transverse and propagation direction gradients.

Deﬁne the propagation direction gradient as e3∂z, and transverse gradient by

∇t = ∇ − e3∂z.

Given this deﬁnition, we seek to show that

Theorem 3.21: Transverse and propagation ﬁeld solutions.

Given a ﬁeld propagating along the z-axis (either forward or backwards), with angular frequency ω, represented by the real part of

F(x, y, z, t) = F(x, y)e jωt∓ jkz,

the ﬁeld components that solve the source free Maxwell’s equation are related by

1 Ft = j ω ∇tFz c ∓ ke3 1 Fz = j ω ∇tFt. c ∓ ke3 Written out explicitly, the transverse ﬁeld component expands as

j ωη Et = ±k∇tEz + e3 × ∇tHz ω 2 2 c c − k j ω ηHt = ±kη∇tHz − e3 × ∇tEz . ω 2 2 c c − k 194 electromagnetism.

To prove we ﬁrst insert the assumed phasor representation into Maxwell’s equation, which gives ω ∇ + j ∓ ke F(x, y) = 0. (3.206) t c 3 Dropping the x, y dependence for now (i.e. F(x, y) → F, we ﬁnd a relation between the transverse gradient of F and the propagation direction gradient of F ω ∇ F = − j ∓ ke F. (3.207) t c 3

From this we now seek to determine the relationships between Ft and Fz. Since ∇t has no xˆ, yˆ components, e3 anticommutes with the transverse gradient

e3∇t = −∇te3, (3.208)

but commutes with 1 ∓ e3. This means that

1 1 (∇tF ± e3 (∇tF) e3) = (∇tF ∓ ∇te3Fe3) 2 2 (3.209) 1 = ∇ (F ∓ e Fe ) , t 2 3 3 or 1 (∇tF + e3 (∇tF) e3) = ∇tFt 2 (3.210) 1 (∇ F − e (∇ F) e ) = ∇ F , 2 t 3 t 3 t z so Maxwell’s equation eq. (3.207) becomes ω ∇ F = − j ∓ ke F t t c 3 z ω (3.211) ∇ F = − j ∓ ke F . t z c 3 t Provided ω2 , (kc)2, these can be inverted. Such an inversion allows an application of the transverse gradient to whichever one of Fz, Ft is known, to compute the other, as stated in theorem 3.21. The relation for Ft in theorem 3.21 is usually stated in terms of the electric and magnetic ﬁelds. To perform that expansion, we must ﬁrst evaluate the multivector inverse explicitly ω ± ke3 F = j c ∇ F z 2 t t ω 2 c − k ω (3.212) ± ke3 F = j c ∇ F . t 2 t z ω 2 c − k 3.11 multivector potential. 195 so that we are in position to expand most of the terms in the numerator

ω ω ± ke ∇ F = − e ± k ∇ e F c 3 t z 3 c t 3 z ω = ±k − e ∇ (E + IηH ) (3.213) 3 c t z z ωη ω = ±k∇ E + e × ∇ H + I ±kη∇ H − e × ∇ E , t z c 3 t z t z c 3 t z from which the transverse electric and magnetic ﬁelds stated in theorem 3.21 can be read oﬀ.A similar expansion for Ez, Hz in terms of Et, Ht is also possible.

Exercise 3.8 Transverse electric and magnetic ﬁeld components. Fill in the missing details in the steps of eq. (3.213).

Exercise 3.9 Propagation direction components.

Perform an expansion like eq. (3.213) to ﬁnd Ez, Hz in terms of Et, Ht.

3.11 multivector potential.

3.11.1 Deﬁnition.

Conventional electromagnetism utilizes scalar and vector potentials, so it is reasonable to expect that the desired multivector representation of the potential is a grade 0,1 multivector. A potential representation with grades 2,3 works for (ﬁctitious) magnetic sources, so we may generally allow a multivector potential to have any grades. Such a potential is related to the ﬁeld as follows.

Deﬁnition 3.15: Multivector potential.

The electromagnetic ﬁeld strength F for a multivector potential A is * ! + 1 ∂ F = ∇ − A . c ∂t 1,2

1 ∂ Before unpacking ∇ − c ∂t A, we want to label the diﬀerent grades of the multivector potential, and do so in a way that is consistent with the conventional potential representation of the electric and magnetic ﬁelds. 196 electromagnetism.

Deﬁnition 3.16: Multivector potential representation.

Let

A = −φ + cA + ηI (−φm + cF) ,

where

1. φ is the scalar potential V (Volts).

2. A is the vector potential W/m (Webers/meter).

3. φm is the scalar potential for (ﬁctitious) magnetic sources A (Amperes).

4. F is the vector potential for (ﬁctitious) magnetic sources C (Coulombs).

This specific breakdown of A into scalar and vector potentials, and dual (pseudoscalar and bivector) potentials has been chosen to match SI conventions, specifically those of [3] (which includes fictitious magnetic sources.) We can now express the fields in terms of the potentials.

Theorem 3.22: Fields and the potential wave equations.

In terms of the potential components, the electric ﬁeld vector and the magnetic ﬁeld bivector are * ! + 1 ∂ ∂A 1 E = ∇ − A = −∇φ − − ∇ × F c ∂t 1 ∂t * ! + ! 1 ∂ ∂F 1 IηH = ∇ − A = Iη −∇φm − + ∇ × A . c ∂t 2 ∂t µ 3.11 multivector potential. 197

The potentials are related to the sources by ! ρ ∂ 1 ∂φ φ = − − ∇ · A + ∂t c2 ∂t ! 1 ∂φ A = −µJ + ∇ ∇ · A + c2 ∂t ! 1 ∂φ F = −M + ∇ ∇ · F + m c2 ∂t ! ρ ∂ 1 ∂φ φ = − m − ∇ · F + m m µ ∂t c2 ∂t

To prove theorem 3.22 we start by expanding (∇ − (1/c)∂t)A using definition 3.16 and then group by grade to find ! ! 1 ∂ 1 ∂ ∇ − A = ∇ − (−φ + cA + ηI (−φ + cF)) c ∂t c ∂t m 1 ∂φ ∂A = −∇φ + c∇ · A + c∇ ∧ A + − c ∂t ∂t ! 1 ∂φ ∂F + Iη −∇φ + c∇ · F + c∇ ∧ F + m − m c ∂t ∂t 1 ∂φ = c∇ · A + (3.214) c ∂t ! ∂A 1 ∂F 1 + −∇φ − − ∇ × F + Iη −∇φ − + ∇ × A ∂t m ∂t µ E IηH ! 1 ∂φ + Iη c∇ · F + m , c ∂t which shows the claimed field split. 1 ∂ In terms of the potentials Maxwell’s equation ∇ + c ∂t F = J is ! * ! + 1 ∂ 1 ∂ ∇ + ∇ − A = J, (3.215) c ∂t c ∂t 1,2 or ! * ! + 1 ∂ 1 ∂ A = J + ∇ + ∇ − A . (3.216) c ∂t c ∂t 0,3 198 electromagnetism.

This is almost a wave equation. Inserting eq. (3.214) into eq. (3.216) and selecting each grade gives four almost-wave equations ! ρ 1 ∂ 1 ∂φ − φ = + c∇ · A + c ∂t c ∂t ! 1 ∂φ c A = −ηJ + ∇ c∇ · A + c ∂t !! 1 ∂φ ηcI F = −IM + ∇ · Iη c∇ · F + m c ∂t ! 1 ∂ 1 ∂φ −Iη φ = Icρ + Iη c∇ · F + m m m c ∂t c ∂t

Using η = µc, ηc = 1, and ∇ · (Iψ) = I∇ψ for scalar ψ, a bit of rearrangement completes the proof.

3.11.2 Gauge transformations.

2 2 Clearly it is desirable if potentials can be found for which ∇ · A + (1/c )∂tφ = ∇ · F + (1/c )∂tφm = 0. Finding such potentials relies on the fact that the potential representation is not unique. In particular, we have the freedom to add any spacetime gradient of any scalar or pseudoscalar potential without changing the ﬁeld.

Theorem 3.23: Gauge invariance.

The spacetime gradient of a grade 0,3 multivector Ψ may be added to a multivector potential ! 1 ∂ A0 = A + ∇ + Ψ, c ∂t

without changing the ﬁeld. That is * ! + * ! + 1 ∂ 1 ∂ F = ∇ − A = ∇ − A0 . c ∂t 1,2 c ∂t 1,2

To prove theorem 3.23 let ! 1 ∂ A0 = A + ∇ + (ψ + Iφ), (3.217) c ∂t 3.11 multivector potential. 199 where ψ and φ are scalar functions. The ﬁeld for potential A0 is

* ! + 1 ∂ F0 = ∇ − A0 c ∂t 1,2 * ! ! !+ 1 ∂ 1 ∂ = ∇ − A + ∇ + (ψ + Iφ) (3.218) c ∂t c ∂t 1,2 * ! + * ! ! + 1 ∂ 1 ∂ 1 ∂ = ∇ − A + ∇ − ∇ + (ψ + Iφ) c ∂t 1,2 c ∂t c ∂t 1,2 = F + h(ψ + Iφ)i1,2, which is just F since since the d’Lambertian operator is a scalar operator and ψ + Iφ has no vector nor bivector grades. 1 ∂ We say that we are working in the Lorenz gauge, if the 0,3 grades of ∇ − c ∂t A are zero, or a transformation that kills those grades is made.

Theorem 3.24: Lorentz gauge transformation.

Given any multivector potential A solution of Maxwell’s equation, the transformation ! 1 ∂ A0 = A − ∇ + Ψ, c ∂t

where * ! + 1 ∂ Ψ = ∇ − A , c ∂t 0,3 allows Maxwell’s equation to be written in wave equation form

0 A = J.

A potential satisfying this wave equation is said to be in the Lorentz gauge.

To prove theorem 3.24, let ! 1 ∂ A = A0 + ∇ + Ψ, (3.219) c ∂t 200 electromagnetism.

so Maxwell’s equation becomes

! * ! + 1 ∂ 1 ∂ J = ∇ + ∇ − A c ∂t c ∂t 1,2 ! * ! + 1 ∂ 1 ∂ = A − ∇ + ∇ − A c ∂t c ∂t 0,3 ! ! * ! + (3.220) 0 1 ∂ 1 ∂ 1 ∂ = A + ∇ + Ψ − ∇ + ∇ − A c ∂t c ∂t c ∂t 0,3 !  * ! +  0 1 ∂  1 ∂  = A + ∇ + Ψ − ∇ − A  . c ∂t c ∂t 0,3 Requiring * ! + 1 ∂ Ψ = ∇ − A , (3.221) c ∂t 0,3

completes the proof. Observe that Ψ has only grades 0,3 as required of a gauge function. Such a transformation completely decouples Maxwell’s equation, providing one scalar wave 0 0 equation for each grade of A = J, relating each grade of the potential A to exactly one grade of the source multivector current J. We are free to immediately solve for A0 using the (causal) Green’s function for the d’Lambertian

Z δ(|x − x0| − c(t − t0) A0(x, t) = − dV0dt0 J(x0, t0) 4π kx − x0k (3.222) 1 Z J(x0, t − 1 kx − x0k) = − dV0 c , 4π kx − x0k which is the sum of all the current contributions relative to the point x at the retarded time 0 tr = t − (1/c) kx − x k. The field follows immediately by differentiation and grade selection * ! + 1 ∂ F = ∇ − A0 . (3.223) c ∂t 1,2 Again, using the Green’s function for the d’Lambertian, the explicit form of the gauge function Ψ is D E Z ∇ − 1 ∂ A(x0, t ) 1 c ∂t r 0,3 Ψ = − dV0 , (3.224) 4π kx − x0k however, we don’t actually need to compute this. Instead, we only have to know we are free to 0 0 construct a field from any solution A of A = J using eq. (3.223). 3.11 multivector potential. 201

3.11.3 Far ﬁeld.

Theorem 3.25: Far ﬁeld magnetic vector potential.

Given a vector potential with a radial spherical wave representation

e− jkr A = A(θ, φ), r the far ﬁeld (r 1) electromagnetic ﬁeld is

F = − jω (1 + rˆ)(rˆ ∧ A) .

If A⊥ = rˆ (rˆ ∧ A) represents the non-radial component of the potential, the respective electric and magnetic ﬁeld components are

E = − jωA⊥ 1 H = rˆ × E. η

To prove theorem 3.25, we will utilize a spherical representation of the gradient

∇ = rˆ∂r + ∇⊥ θˆ φˆ (3.225) ∇⊥ = ∂ + ∂ . r θ r sin θ φ The gradient of the vector potential is

e− jkr ∇A = (rˆ∂ + ∇⊥) A r r ! 1 e− jkr e− jkr = rˆ − jk − A + ∇⊥A r r r (3.226) ! 1 = − jk + rAˆ + O(1/r2) r ≈ − jkrAˆ .

Here, all the O(1/r2) terms, including the action of the non-radial component of the gradient on the 1/r potential, have been neglected. From eq. (3.226) the far ﬁeld divergence and the (bivector) curl of A are ∇ · A = − jkrˆ · A (3.227) ∇ ∧ A = − jkrˆ ∧ A. 202 electromagnetism.

Finally, the far ﬁeld gradient of the divergence of A is

∇ (∇ · A) = (rˆ∂r + ∇⊥) (− jkrˆ · A) ≈ − jkrˆ∂r (rˆ · A) ! 1 (3.228) = − jkrˆ − jk − (rˆ · A) r ≈ −k2rˆ (rˆ · A) ,

again neglecting any O(1/r2) terms. The ﬁeld is

c2 F = − jωA − j ∇ (∇ · A) + c∇ ∧ A ω − jωA jωr (r · A) − jkcr ∧ A = + ˆ ˆ ˆ (3.229) = − jω (A − rˆ (rˆ · A)) − jωrˆ ∧ A = − jωrˆ (rˆ ∧ A) − jωrˆ ∧ A = − jω (rˆ + 1)(rˆ ∧ A) ,

which completes the first part of the proof. Extraction of the electric and magnetic fields can be done by inspection and is left to the reader to prove. One interpretation of this is that the (bivector) magnetic field is represented by the plane perpendicular to the direction of propagation, and the electric field by a vector in that plane.

Theorem 3.26: Far ﬁeld electric vector potential.

Given a vector potential with a radial spherical wave representation

e− jkr F = F(θ, φ), r the far ﬁeld (r 1) electromagnetic ﬁeld is

F = − jωηI (rˆ + 1)(rˆ ∧ F) .

If F⊥ = rˆ (rˆ ∧ F) represents the non-radial component of the potential, the respective electric and magnetic ﬁeld components are

E = jωηrˆ × F

H = − jωF⊥.

The proof of theorem 3.26 is left to the reader. 3.11 multivector potential. 203

Example 3.1: Vertical dipole potential.

We will calculate the far ﬁeld along the propagation direction vector kˆ in the z-y plane

iθ kˆ = e3e (3.230) i = e32, for the inﬁnitesimal dipole potential e µI l A = 3 0 e− jkr, (3.231) 4πr as illustrated in ﬁg. 3.11.

Figure 3.11: Vertical inﬁnitesimal dipole and selected propagation direction.

The wedge of kˆ with A is proportional to

D E kˆ ∧ e = keˆ 3 3 2 D iθ E = e3e e3 (3.232) D E 2 = e2e−iθ 3 2 = −i sin θ, so from theorem 3.26 the ﬁeld is µI l F = jω 1 + e eiθ i sin θ 0 e− jkr. (3.233) 3 4πr 204 electromagnetism.

The electric and magnetic ﬁelds can be found from the respective vector and bivector grades of eq. (3.233)

jωµI l E = 0 e− jkre eiθi sin θ 4πr 3 jωµI l = 0 e− jkre eiθ sin θ (3.234) 4πr 2 jkηI l sin θ = 0 e− jkr (e cos θ − e sin θ) , 4πr 2 3 and

1 µI l H = jωi sin θ 0 e− jkr Iη 0 4πr 1 µI l = e e jω sin θ 0 e− jkr (3.235) η 321 32 0 4πr jk sin θ I l = −e 0 0 e− jkr. 1 4πr The multivector electrodynamic field expression eq. (3.233) for F is more algebraically compact than the separate electric and magnetic field expressions, but this comes with the complexity of dealing with different types of imaginaries. There are two explicit unit imaginaries in eq. (3.233), the scalar imaginary j used to encode the time harmonic nature of the field, and i = e32 used to represent the plane that the far field propagation direction vector lay in. Additionally, when the magnetic field component was extracted, the pseudoscalar I = e123 entered into the mix. Care is required to keep these all separate, especially since I, j commute with all grades, but i does not.

3.12 dielectric and magnetic media.

3.12.1 Statement.

Without imposing the constitutive relationships eq. (3.2) the geometric algebra form of Maxwell’s equations requires a pair of equations, multivector ﬁelds, and multivector sources, instead of one of each.

Theorem 3.27: Maxwell’s equations in media. 3.12 dielectric and magnetic media. 205

Maxwell’s equations in media are * ! + 1 ∂ ∇ + F = Je c ∂t 0,1 * ! + 1 ∂ ∇ + G = IJm, c ∂t 2,3 where c is the group velocity of F, G in the medium, the ﬁelds are grade 1,2 multivectors

I F = D + H c G = E + IcB,

and the sources are grade 0,1 multivectors

1 J = ρ − J e c Jm = cρm − M.

To prove theorem 3.27 we may simply expand the spacetime gradients and grade selection operations, and compare to eq. (3.1), the conventional representation of Maxwell’s equations. For F we have

* ! + J 1 ∂ ρ − = ∇ + F c c ∂t 0,1 * ! + 1 ∂ I = ∇ + D + H c ∂t c 0,1 (3.236) * + I I 1 ∂D 1 ∂H = ∇ · D + ∇ ∧ D + ∇ · H + ∇ ∧ H + + I 2 c c c ∂t c ∂t 0,1 1 ∂D 1 = ∇ · D + − ∇ × H, c ∂t c 206 electromagnetism.

and for G * ! + 1 ∂ I (cρm − M) = ∇ + G c ∂t 2,3 * ! + 1 ∂ = ∇ + (E + IcB) c ∂t 2,3 * + 1 ∂E ∂B = ∇ · E + ∇ ∧ E + Ic∇ · B + Ic∇ ∧ B + + I (3.237) c ∂t ∂t 2,3 ∂B = ∇ ∧ E + Ic∇ · B + I ∂t ! ∂B = I ∇ × E + c∇ · B + . ∂t Applying further grade selection operations, rescaling (cancelling all factors of c and I), and a bit of rearranging, gives ∇ · D = ρ ∂D ∇ × H = J + ∂t (3.238) ∇ · B = ρm ∂B ∇ × E = −M − , ∂t which are Maxwell’s equations, completing the proof.

Exercise 3.10 Maxwell’s equations in media. The proof above is somewhat unfriendly, as it works backwards from the answer. No motivation was given for why the particular multivector ﬁelds were chosen, nor why grade selection operations were required. To obtain some insight on why this works, prove theorem 3.27 from eq. (3.2) directly as follows: 1. Eliminate cross products using ∇ × f = I(∇ ∧ f).

2. Introduce a scalar constant c with dimensions of velocity and redimensionalize any time derivatives ∂f/∂t = (1/c)∂(cf)/∂t, so that [(1/c)∂/∂t] = [∇].

3. If required, multiply each of Maxwell’s equations by a factor of I, to obtain a scalar and vector equation for D, H, and a bivector and pseudoscalar equation for E, B.

4. Sum the pairs of equations to form a multivector equation for each of D, H and E, B.

5. Factor the terms in each equation into a product of the spacetime gradient and the respective ﬁelds F, G, and show the result may be simpliﬁed by grade selection. 3.12 dielectric and magnetic media. 207

3.12.2 Alternative form.

Theorem 3.28: Grade selection free equations.

Given multivector solutions F0, G0 to ! 1 ∂ J = ∇ + F0 e c ∂t ! 1 ∂ IJ = ∇ + G0, m c ∂t

these can be related to solutions F, G of Maxwell’s equations given by theorem 3.27 by

0 F = F 1,2 0 G = G 1,2,

if * ! + 1 ∂ ∇ + F0 = 0 c ∂t 0,1 * ! + 1 ∂ 0 ∇ + G 3 = 0. c ∂t 2,3

To prove we select the grade 0,1 and grade 2,3 components from space time gradient equations of theorem 3.28. For the electric sources, this gives * ! + 1 ∂ 0 Je = ∇ + F c ∂t 0,1 * ! + * ! + * ! + (3.239) 1 ∂ 0 1 ∂ 0 1 ∂ 0 = ∇ + F 1,2 + ∇ + F + ∇ + F 3 , c ∂t 0,1 c ∂t 0,1 c ∂t 0,1 1 ∂ 0 however ∇ + c ∂t hF i3 has only grade 2,3 components, leaving just * ! + * ! + 1 ∂ 0 1 ∂ 0 Je = ∇ + F 1,2 + ∇ + F , (3.240) c ∂t 0,1 c ∂t 0,1 as claimed. For the magnetic sources, we have * ! + 1 ∂ 0 IJm = ∇ + G c ∂t 2,3 * ! + * ! + * ! + (3.241) 1 ∂ 0 1 ∂ 0 1 ∂ 0 = ∇ + G 1,2 + ∇ + G + ∇ + G 3 , c ∂t 2,3 c ∂t 2,3 c ∂t 2,3 208 electromagnetism.

1 ∂ 0 however ∇ + c ∂t hG i0 has only grade 0,1 components, leaving just * ! + * ! + 1 ∂ 0 1 ∂ 0 IJm = ∇ + G 1,2 + ∇ + G , (3.242) c ∂t 2,3 c ∂t 2,3 completing the proof. Theorem 3.28 is probably a more eﬀect geometric algebra form for solution of Maxwell’s equations in matter, as the grade selection free spacetime gradients can be solved for F0, G0 directly using Green’s function convolution. However, we have an open question of how to impose a zero scalar grade constraint on F0 and a zero pseudoscalar grade constraint on G0.

Question: Is the solution as simple as grade selection of the convolution? Z 0 0 0 0 F = dt dV G(x − x , t − t )Je 1,2 Z (3.243) 0 0 0 0 G = dt dV G(x − x , t − t )IJm 1,2,

where G(x − x0, t − t0), is the Green’s function for the space time gradient theorem 2.19, not to be confused with G = E + IcB,

3.12.3 Gauge like transformations.

Because of the grade selection operations in theorem 3.27, we cannot simply solve for F, G using the Green’s function for the spacetime gradient. However, we may make a gauge-like transformation of the ﬁelds. Additional exploration is required to determine if such transformations can be utilized to solve theorem 3.27.

Theorem 3.29: Multivector transformation of the ﬁelds.

If F, G are solutions to theorem 3.27, then so are * ! + 0 1 ∂ F = F + ∇ − Ψ2,3 c ∂t 1,2 * ! + 0 1 ∂ G = G + ∇ − Ψ0,1 , c ∂t 1,2

where Ψ2,3 is any multivector with grades 2,3 and Ψ0,1 is any multivector with grades 0,1. 3.12 dielectric and magnetic media. 209

To prove theorem 3.29 we need to show that * ! + * ! + 1 ∂ 1 ∂ ∇ + F0 = ∇ + F c ∂t 0,1 c ∂t 0,1 * ! + * ! + (3.244) 1 ∂ 1 ∂ ∇ + G0 = ∇ + G . c ∂t 2,3 c ∂t 2,3 Let’s start with F * ! + * ! + * ! * ! + + 1 ∂ 1 ∂ 1 ∂ 1 ∂ ∇ + F0 = ∇ + F + ∇ + ∇ − Ψ c ∂t c ∂t c ∂t c ∂t 2,3 0,1 0,1 1,2 0,1 * ! + 1 ∂ = ∇ + F + Ψ2,3 0,1 (3.245) c ∂t 0,1 * ! * ! + + 1 ∂ 1 ∂ − ∇ + ∇ − Ψ . c ∂t c ∂t 2,3 0,3 0,1

The second term is killed since Ψ2,3 has no grade 0,1 components by definition, so neither 1 ∂ does Ψ2,3. To see that the last term is zero, note that ∇ − Ψ2,3 can have only grades D E c ∂t D E 1,2,3, so ∇ − 1 ∂ Ψ is a trivector. This means that ∇ + 1 ∂ ∇ − 1 ∂ Ψ has c ∂t 2,3 0,3 c ∂t c ∂t 2,3 0,3 only grades 2,3, which are obliterated by the final grade 0,1 selection operation, leaving just D E ∇ + 1 ∂ F . For G we have c ∂t 0,1 * ! + * ! + * ! * ! + + 1 ∂ 1 ∂ 1 ∂ 1 ∂ ∇ + G0 = ∇ + G + ∇ + ∇ − Ψ c ∂t c ∂t c ∂t c ∂t 0,1 2,3 2,3 1,2 2,3 * ! + 1 ∂ = ∇ + G + Ψ0,1 2,3 (3.246) c ∂t 2,3 * ! * ! + + 1 ∂ 1 ∂ − ∇ + ∇ − Ψ . c ∂t c ∂t 0,1 0,3 2,3 As before the d’Lambertian term is killed as it has no grades 2,3. To see that the last term is D E zero, note that ∇ − 1 ∂ Ψ can have only grades 0,1,2, so ∇ − 1 ∂ Ψ is a scalar. This c ∂t 0,1 c ∂t 0,1 0,3 1 ∂ D 1 ∂ E means that ∇ + c ∂t ∇ − c ∂t Ψ0,1 has only grades 0,1, which are obliterated by the final 0D,3 E grade 2,3 selection operation, leaving ∇ + 1 ∂ G , completing the proof. c ∂t 2,3 An additional variation of theorem 3.29 is also possible.

Theorem 3.30: Multivector transformation of the ﬁelds. 210 electromagnetism.

If F, G are solutions to theorem 3.27, then so are ! 1 ∂ F0 = F + ∇ − Ψ c ∂t 2,3 ! 1 ∂ G0 = G + ∇ − Ψ c ∂t 0,1

where Ψ2,3 is any multivector with grades 2,3 and Ψ0,1 is any multivector with grades 0,1.

Theorem 3.30 can be proven by direct substitution. For F

* ! ! !+ * ! + 1 ∂ 1 ∂ 1 ∂ ∇ + F + ∇ − Ψ2,3 = ∇ + F + Ψ2,3 c ∂t c ∂t 0,1 c ∂t 0,1 * ! + (3.247) 1 ∂ = ∇ + F c ∂t , and for G

* ! ! !+ * ! + 1 ∂ 1 ∂ 1 ∂ ∇ + G + ∇ − Ψ0,1 = ∇ + G + Ψ0,1 c ∂t c ∂t 2,3 c ∂t 2,3 * ! + (3.248) 1 ∂ = ∇ + G c ∂t , which completes the proof.

3.12.4 Boundary value conditions.

Theorem 3.31: Boundary value relations.

The diﬀerence in the normal and tangential components of the electromagnetic ﬁeld spanning a surface on which there are a surface current or surface charge or current densities Je = Jesδ(n), Jm = Jmsδ(n) can be related to those surface sources as follows

hnˆ(F2 − F1)i0,1 = Jes

hnˆ(G2 − G1)i2,3 = IJms, 3.12 dielectric and magnetic media. 211

where Fk = Dk + IHk/c, Gk = Ek + IcBk, k = 1, 2 are the ﬁelds in the where nˆ = nˆ 2 = −nˆ 1 is the outwards facing normal in the second medium. In terms of the conventional constituent ﬁelds, these may be written

nˆ · (D2 − D1) = ρs

nˆ × (H2 − H1) = Js

nˆ · (B2 − B1) = ρms

nˆ × (E2 − E1) = −Ms.

Figure 3.12 illustrates a surface where we seek to find the fields above the surface (region 2), and below the surface (region 1). These fields will be determined by integrating Maxwell’s equation over the pillbox configuration, allowing the height n of that pillbox above or below the surface to tend to zero, and the area of the pillbox top to also tend to zero.

Figure 3.12: Pillbox integration volume.

We will work with theorem 3.27, Maxwell’s equations in media, in their frequency domain form

h∇Fi0,1 + jkD = Jesδ(n) (3.249) h∇Gi2,3 + jkIcB = IJmsδ(n), and integrate these over the pillbox volume in the ﬁgure. That is Z Z Z dVh∇Fi0,1 + jk dVD = dndAJesδ(n) Z Z Z (3.250) dVh∇Gi2,3 + jkIc dVB = I dndAJmsδ(n). 212 electromagnetism.

The gradient integrals can be evaluated with theorem 2.11. Evaluating the delta functions picks leaves an area integral on the surface. Additionally, we assume that we are making the pillbox volume small enough that we can employ the mean value theorem for the D, B integrals Z dAhnˆ Fi0,1 + jk∆A n1D˜ 1 + n2D˜ 2 = ∆AJes ∂V (3.251) Z dAhnˆGi2,3 + jkIc∆A n1B˜ 1 + n2B˜ 2 = I∆AJms. ∂V

We now let n1, n2 tend to zero, which kills off the D, B contributions, and also kills off the side wall contributions in the first pillbox surface integral. This leaves

hnˆ 2F2i0,1 + hnˆ 1F1i0,1 = Jes (3.252) hnˆ 2G2i2,3 + hnˆ 1G1i2,3 = Jms.

Inserting nˆ = nˆ 2 = −nˆ 1 completes the ﬁrst part of the proof. Expanding the grade selection operations, we ﬁnd

nˆ · (D2 − D1) = ρs

Inˆ ∧ (H2/c − H1/c) = −Js/c (3.253) nˆ ∧ (E2 − E1) = −IMs

Icnˆ · (B2 − B1) = Icρms,

and expansion of the wedge’s as cross’s using eq. (1.58) completes the proof. In the special case where there are surface charge and current densities along the interface surface, but the media is uniform (1 = 2, µ1 = µ2), then the ﬁeld and current relationship has a particularly simple form [5]

nˆ(F2 − F1) = Js. (3.254)

Exercise 3.11 Uniform media with currents and densities.

Prove that eq. (3.254) holds when 1 = 2, µ1 = µ2. DISTRIBUTIONTHEOREMS. A

Theorem A.1: Vector Blade dot and wedge product relations.

Given a k-blade B and a vector a, the dot and wedge products have the following commutation relationships

B · a = (−1)k−1a · B (A.1) B ∧ a = (−1)ka ∧ B,

and can be expressed as symmetric and antisymmetric sums depending on the grade of the blade

1 a ∧ B = aB + (−1)kBa 2 (A.2) 1 a · B = aB − (−1)kBa . 2

To prove these, split the blade into components that intersect with and are disjoint from a as follows 1 B = n n ··· n + m m ··· m , (A.3) a 1 2 k−1 1 2 k where ni are all mutually normal and normal to a and mi are all normal. The products of B with a are

1 aB = a n n ··· n + am m ··· m a 1 2 k−1 1 2 k (A.4) = n1n2 ··· nk−1 + am1m2 ··· mk, and

1 Ba = n n ··· n a + m m ··· m a a 1 2 k−1 1 2 k k−1 k (A.5) = (−1) n1n2 ··· nk−1 + (−1) am1m2 ··· mk k = (−1) (−n1n2 ··· nk−1 + am1m2 ··· mk) ,

213 214 distribution theorems.

or k (−1) Ba = −n1n2 ··· nk−1 + am1m2 ··· mk. (A.6)

Respective addition and subtraction of eq. (A.4) and eq. (A.6) gives

k aB + (−1) Ba = 2am1m2 ··· mk (A.7) = 2a ∧ B,

and

k aB − (−1) Ba = 2n1n2 ··· nk−1 (A.8) = 2a · B,

proving eq. (A.2). Grade selection from eq. (A.6) gives

k (−1) B · a = −n1n2 ··· nk−1 (A.9) = −a · B,

and

k (−1) B ∧ a = am1m2 ··· mk (A.10) = a ∧ B,

which proves eq. (A.1).

Theorem A.2: Vector-trivector dot product.

Given a vector a and a blade b ∧ c ∧ d formed by wedging three vectors, the dot product of the two can be expanded as bivectors like

· ∧ ∧ ∧ ∧ · a (b c d) = (b c d) a (A.11) = (a · b)(c ∧ d) − (a · c)(b ∧ d) + (a · d)(b ∧ c).

The proof follows by expansion in coordinates X D E a · (b ∧ c ∧ d) = aib jckdl eie jekel . (A.12) 2 j,k,l The products within the grade two selection operator can be of either grade two or grade four, so only the terms where one of i = j, i = k, or i = l contributes. Repeated anticommutation of distribution theorems. 215 the normal unit vectors can put each such pair adjacent, where they square to unity. Those are respectively

heieiekeli2 = ekel D E D E e e e e = − e e e e = −e e i j i l 2 j i i l 2 j l (A.13) D E D E D E eie jekei = − e jeiekei = + e jekeiei = e jek. 2 2 2 Substitution back into eq. (1.83) gives

X a · (b ∧ c ∧ d) = aib jckdl ei · e j(ekel) − ei · ek(e jel) + ei · el(e jek) j,k,l (A.14) = (a · b)(c ∧ d) − (a · c)(b ∧ d) + (a · d)(b ∧ c).

Theorem A.2 is a speciﬁc case of the more general identity

Theorem A.3: Vector blade dot product distribution.

A vector dotted with a n − blade distributes as

n X i x · (y1 ∧ y2 ∧ · · · ∧ yn) = (−1) (x · yi) (y1 ∧ · · · ∧ yi−1 ∧ yi+1 ∧ · · · ∧ yn) . i=1 This dot product is symmetric(antisymmetric) when the grade of the blade the vector is dotted with is odd(even).

For a proof of theorem A.3 (valid for all metrics) see [6].

Theorem A.4: Distribution of inner products

Given two blades As, Br with grades subject to s > r > 0, and a vector b, the inner product distributes according to

As · (b ∧ Br) = (As · b) · Br.

The proof is straightforward, but also mechanical. Start by expanding the wedge and dot products within a grade selection operator

As · (b ∧ Br) = hAs(b ∧ Br)is−(r+1) 1 (A.15) = A bB + (−1)r B b . 2 s r r s−(r+1) 216 distribution theorems.

Solving for Brb in r 2b · Br = bBr − (−1) Brb, (A.16)

we have

1 A · (b ∧ B ) = hA bB + A (bB − 2b · B )i s r 2 s r s r r s−(r+1) (A.17) ((( h i − (· (( = AsbBr s−(r+1) (A(s ((b Br) s−(r+1). The last term above is zero since we are selecting the s − r − 1 grade element of a multivector with grades s − r + 1 and s + r − 1, which has no terms for r > 0. Now we can expand the Asb multivector product, for

As · (b ∧ Br) = h(As · b + As ∧ b) Bris−(r+1). (A.18)

The latter multivector (with the wedge product factor) above has grades s + 1 − r and s + 1 + r, so this selection operator ﬁnds nothing. This leaves

As · (b ∧ Br) = h(As · b) · Br + (As · b) ∧ Bris−(r+1). (A.19)

The ﬁrst dot products term has grade s − 1 − r and is selected, whereas the wedge term has grade s − 1 + r , s − r − 1 (for r > 0). PROOFSKETCHFORTHEFUNDAMENTALTHEOREMOF B GEOMETRICCALCULUS.

We start with expanding the hypervolume integral, by separating the geometric product of the volume element and vector derivative direction vectors into dot and wedge contributions

Z ↔ Z ↔ k X k i Fd x ∂ G = d uFIkx ∂ i G V V i (B.1) Z ↔ X k i i = d uF Ik · x + Ik ∧ x ∂ i G. i V

i n o Because x lies in span x j , the wedge product above is zero, leaving

Z ↔ Z ↔ k X k i Fd x ∂ G = d uF Ik · x ∂ i G, V i V Z Z X k i X k i = d u(∂iF)Ik · x G + d uF Ik · x (∂iG) (B.2) i V i V   X Z Z X  k · i − k  · i  = d u∂i F Ik x G d uF  ∂i Ik x  G. i V V i The sum in the second integral turns out to be zero, but is somewhat messy to show in general. The k = 1 is a special case, as it is trivial

1 ∂1(x1 · x ) = ∂11 = 0. (B.3)

The k = 2 case is illustrative

2 X i 1 2 ∂i I3 · x = ∂1((x1 ∧ x2) · x ) + ∂2((x1 ∧ x2) · x ) i =1 (B.4) = ∂1(−x2) + ∂2x1 ∂2x ∂2x = − + , ∂u1∂2 ∂u2∂1

217 218 proof sketch for the fundamental theorem of geometric calculus.

which is zero by equality of mixed partials. To show that this sums to zero in general observe that cyclic permutation of the wedge factors in the pseudoscalar only changes the sign

1(k−1) x1 ∧ x2 ∧ · · · ∧ xk = x2 ∧ x3 ∧ · · · ∧ xk ∧ x1(−1) 2(k−1) (B.5) = x3 ∧ x4 ∧ · · · ∧ xk ∧ x1 ∧ x2(−1) i(k−1) = xi+1 ∧ xi+2 ∧ · · · ∧ xk ∧ x1 ∧ x2 ∧ · · · ∧ xi(−1) .

i The pseudoscalar dot product Ik · x is therefore

i i Ik · x = (x1 ∧ x2 ∧ · · · ∧ xk) · x (B.6) i(k−1) = xi+1 ∧ xi+2 ∧ · · · ∧ xk ∧ x1 ∧ x2 ∧ · · · ∧ xi−1(−1) ,

and the sum is

X i ∂i Ik · x i i(k−1) = (∂i,i+1x) ∧ xi+2 ∧ · · · ∧ xk ∧ x1 ∧ x2 ∧ · · · ∧ xi−1(−1) i(k−1) + xi+1 ∧ (∂i,i+2x) ∧ · · · ∧ xk ∧ x1 ∧ x2 ∧ · · · ∧ xi−1(−1) (B.7) . + . i(k−1) + xi+1 ∧ xi+2 ∧ · · · ∧ xk ∧ x1 ∧ x2 ∧ · · · ∧ (∂i,i−1x)(−1) .

For each i , j there will be one partial ∂i, jx and one partial ∂ j,ix in this sum. Consider, for example, the 1, 2 case which come from the i = 1, 2 terms in the sum

1(k−1) 2(k−1) ∂1(x2 ∧ x3 ∧ · · · ∧ xk−1 ∧ xk)(−1) + ∂2(x3 ∧ x4 ∧ · · · ∧ xk ∧ x1)(−1) 1(k−1) 2(k−1) = (∂1,2x) ∧ x3 ∧ · · · ∧ xk−1 ∧ xk)(−1) + x3 ∧ x4 ∧ · · · ∧ xk ∧ (∂2,1x)(−1) + ··· k−1 k−2 k−1 = (−1) (x3 ∧ · · · ∧ xk−1 ∧ xk) ∧ (−1) ∂1,2x + (−1) ∂2,1x + ··· ! ∂2x ∂2x = (x3 ∧ · · · ∧ xk−1 ∧ xk) ∧ − + + ··· ∂u1∂u2 ∂u2∂u1 (B.8)

By equality of mixed partials this diﬀerence of 1, 2 partials are killed. The same argument holds P i for all other indexes, proving that i ∂i Ik · x = 0. Equation (B.2) is left with a sum of perfect diﬀerentials, each separately integrable

Z ↔ Z Z k X k−1 ∂ i Fd x ∂ G = d ui dui F Ik · x G V ∂V u ∂ui i ∆ i (B.9) Z X k−1 i = d ui F Ik · x G , ∆ui i ∂V proof sketch for the fundamental theorem of geometric calculus. 219 which completes the sketch of the proof. While much of the theoretical heavy lifting was carried by the reciprocal frame vectors, the ﬁnal result does not actually require computing those vectors. When k equals the dimension of the space, as in R3 volume integrals, the vector derivative ∂ is identical to the ∇, in which case we do not even require the reciprocal frame vectors to express the gradient. For a full proof of theorem 2.3, additional mathematical subtleties must be considered. Issues of connectivity of the hypervolumes (and integration theory in general) are covered very nicely in [18]. For other general issues required for a complete proof, like the triangulation of the volume and its boundary, please see [13], [6], and [21].

GREEN’SFUNCTIONS. C c.1 helmholtz operator.

The goal. The Helmholtz equation to solve is ∇2 + k2 f (x) = u(x). (C.1)

To solve using the Green’s function of theorem 2.17, we require ∇2 + k2 G(x, x0) = δ3(x − x0). (C.2)

Verifying this requires two steps, ﬁrst considering points x , x0, and then considering an inﬁnitesimal neighbourhood around x0.

Case I. x , x0. We will absorb the sign associated with the causal and acausal Green’s function variations by writing i = ± j, so that for points x , x0, (i.e. r = kx − x0k , 0), working in spherical coordinates, we ﬁnd

1 −4π ∇2 + k2 G(x, x0) = r2G0 0 − 4πk2G r2 ! ! 1 d ikr 1 k2 = r2 − eikr + eikr r2 dr r r2 r 1 d k2 = (rik − 1) eikr + eikr (C.3) r2 dr r 2 1 ikr k ikr = ik + rik − 1¡ ik e + e r2 r 1 eikr = −rk2 eikr + k2 r2 r = 0.

Case II. In the neighbourhood of kx − x0k < Having shown that we end up with zero ev- erywhere that x , x0 we are left to consider an inﬁnitesimal neighbourhood of the volume surrounding the point x in our integral. Following the Coulomb treatment in §2.2 of [19] we use

221 222 green’s functions.

a spherical volume element centered around x of radius , and then convert a divergence to a surface area to evaluate the integral away from the problematic point.

0 Z 1 Z eikkx−x k ∇2 2 0 0 0 ∇2 2 0 0 + k G(x, x ) f (x )dV = − + k 0 f (x )dV 4π kx−x0k< kx − x k 00 (C.4) 1 Z eikkx k 00 ∇2 2 00 = − f (x + x ) + k 00 dV , 4π kx00k< kx k where a change of variables x00 = x0 − x, as illustrated in ﬁg. C.1, has been performed.

Figure C.1: Neighbourhood kx − x0k < .

We assume that f (x) is suﬃciently continuous and “well behaved” that it can be pulled it out of the integral, replaced with a mean value f (x∗) in the integration neighbourhood around x00 = 0.

00 Z f (x∗) Z eikkx k ∇2 2 0 0 0 ∇2 2 00 + k G(x, x ) f (x )dV = lim − + k 00 dV . (C.5) →0 4π kx00k< kx k C.1 helmholtz operator. 223

The k2 term of eq. (C.5) can be evaluated with a spherical coordinate change of variables

Z ikkx00k Z Z π Z 2π ikr 2 e 00 2 e 2 k 00 dV = k r dr sin θdθdφ kx00k< kx k r=0 θ=0 φ=0 r Z = 4πk2 reikrdr r=0 Z k (C.6) = 4π ueiudu u=0

− iu k = 4π( iu + 1)e 0 = 4π (−ik + 1)eik − 1 .

To evaluate the Laplacian term of eq. (C.5), we can make a change of variables for the Lapla- cian

ikkx00k ikkx00k ikkx00k ! e 2 e e ∇ = ∇ 00 = ∇ 00 · ∇ 00 , (C.7) kx00k x kx00k x x kx00k and then employ the divergence theorem

Z ikkx00k Z ikkx00k ! 2 e 00 e 00 ∇ ∇ 00 ∇ 00 00 dV = x · x 00 dV 00 kx k 00 kx k kx k < kx k< (C.8) Z ikkx00k ! e 00 ∇ 00 = x 00 · nˆdA , ∂V kx k where ∂V represents the surface of the kx00k < neighbourhood, and nˆ is the unit vector directed along x00 = x0 − x. To evaluate this surface integral we will require only the radial portion of the gradient. With r = kx00k, that is

00 ! ! eikkx k ∂ eikr ∇ 00 · nˆ = nˆ · nˆ x kx00k ∂r r ∂ eikr = ∂r r ! (C.9) 1 1 = ik − eikr r r2 eikr = (ikr − 1) . r2 224 green’s functions.

Using spherical coordinates again, with an area element dA00 = r2 sin θdθdφ, we obtain

00 Z eikkx k Z π Z 2π eikr ∇2 00 2 00 dV = (ikr − 1) r sin θdθdφ 00 k k 2 (C.10) kx k < x θ=0 φ=0 r r= = 4π (ik − 1) eik.

Putting everything back together we have

0 1 Z eikkx−x k − ∇2 + k2 f (x0)dV0 = lim − f (x∗) (−ik + 1)eik − 1 + (ik − 1) eik 4π kx − x0k →0 = lim − f (x∗) (−ik + 1 + ik − 1)eik − 1 (C.11) →0 = lim f (x∗). →0 Observe the perfect cancellation of all the explicitly dependent terms. The mean value point x∗ is also dependent, but tends to x in the limit, leaving

0 1 Z eikkx−x k f (x) = − ∇2 + k2 f (x0)dV0. (C.12) 4π kx − x0k

This proves the delta function property that we claimed the Green’s function had.

c.2 delta function derivatives.

The Green’s function for the spacetime gradient ends up with terms like d δ(−r/c + t − t0) dr (C.13) d δ(−r/c + t − t0), dt where t0 is the integration variable of the test function that the delta function will be applied to. If these were derivatives with respect to the integration variable, then we could use Z ∞ ! d 0 0 0 0 δ(t ) φ(t ) = −φ (0), (C.14) −∞ dt which follows by chain rule, and an assumption that φ(t0) is well behaved at the points at inﬁnity. It is not clear that how, if at all, this could be applied to either of eq. (C.13). Let’s go back to square one, and ﬁgure out the meaning of these delta functions by their action on a test function. We wish to compute Z ∞ d δ(au + b − t0) f (t0)dt0. (C.15) −∞ du C.2 delta function derivatives. 225

Let’s start with a change of variables t00 = au + b − t0, for which we ﬁnd

t0 = au + b − t00 00 − 0 dt = dt (C.16) d dt00 d d = = a . du du dt00 dt00 Substitution back into eq. (C.15) gives

Z −∞ ! Z ∞ ! d 00 00 00 d 00 00 00 a 00 δ(t ) f (au + b − t )(−dt ) = a 00 δ(t ) f (au + b − t )dt ∞ dt −∞ dt ∞ 00 − 00 = aδ(t ) f (au + b t ) −∞ Z ∞ 00 d 00 00 − a δ(t ) f (au + b − t )dt (C.17) dt00 −∞ d 00 = −a 00 f (au + b − t ) dt t00=0 d = a f (s) . ds s=au+b This shows that the action of the derivative of the delta function (with respect to a non- integration variable parameter u) is

d 0 d δ(au + b − t ) ∼ a . (C.18) du ds s=au+b

GAELECTRODYNAMICSINTHELITERATURE. D

The notation and nomenclature used to express Maxwell’s equation in the GA literature, much of which has a relativistic focus, has not been standardized. Here is an overview of some of the variations that will be encountered in readings.

Space Time Algebra (STA). [6] Maxwell’s equation is written

∇F = J F = E + IB

I = γ0γ1γ2γ3 (D.1) µ J = γµ J = γ0 (ρ − J) µ ∇ = γ ∂µ = γ0 (∂t + ∇) .

n o µ 2 2 µ STA uses a relativistic basis γµ and its dual {γ } for which γ0 = −γk = 1, k ∈ 1, 2, 3, and γ · µ γν = δ ν. Spatial vectors are expressed in terms of the Pauli basis σi = γiγ0, which are bivectors that behave as Euclidean basis vectors (squaring to unity, and all mutually anticommutative). F is called the electromagnetic ﬁeld strength (and is not a 1,2 multivector, but a bivector), ∇ is called the vector derivative operator, ∇ called the three-dimensional vector derivative operator, and J is called the spacetime current (and is a vector, not a multivector). The physicist’s “natural 2 2 2 units” c = 0 = µ0 are typically used in STA. The d’Lambertian in STA is = ∇ = ∂t − ∇ , although the earliest formulation of STA [10] used for the vector derivative. Only spatial vectors are in bold, and all other multivectors are non-bold. STA is inherently relativistic, and can be used to obtain many of the results in this book more directly. STA can easily be related to the tensor formulation of electrodynamics. Maxwell’s equations as expressed in theorem 3.1 can be converted to their STA form (in SI units) by setting ei = γiγ0 and by left multiplying both sides by γ0.

227 228 ga electrodynamics in the literature.

Algebra of Physical Space (APS). [4] Maxwell’s equation is written as 1 ∂F =  0c F = E + icB i = e123 (D.2) 1 ∂ = ∂ − ∇ c t 1 j = (ρc + j) . 0c F is called the Faraday, ∂ the gradient, j the current density, and 0,1 multivectors are called paravectors. A Euclidean spacial basis {e1, e2, e3} is used, and e0 = 1 is used as the time-like basis “vector”. In APS, where e0 = 1 is not a vector grade object, a standard GA dot product for ν ν which eµ · e = δµ to express proper length. APS uses inner products based on grade selection from the multivector zz, where z is the Cliﬀord conjugation operation that changes the sign of any vector and bivector grades of a multivector z. This conjugation operation is also used to express Lorentz transformations, and is seen in Maxwell’s equation, operating on the current 2 2 2 density and gradient. The d’Lambertian is written as = ∂∂ = (1/c )∂t − ∇ . While APS is only cosmetically diﬀerent than theorem 3.1 the treatment in [4] is inherently relativistic.

Jancewicz. [15] Maxwell’s equation in linear isotropic media is written as √ √ D f + eD ln + bˆD ln µ = ˜ √ ∂ D = ∇ + µ ∂t f = e + bˆ √ e = E (D.3) 1 bˆ = √ IB µ

I = e123 1 √ ˜ = √ ρ − µj. Jancewicz works with fields that have been re-dimensionalized to the same units, uses an overhat bold notation for bivectors (which are sometimes called volutors). D is called the cliffor differential operator, f the electromagnetic cliffor, and ˜the density of electric sources. In media that for which µ, are constant in space and time, his Maxwell equation reduces to D f = ˜. The ∗ 2 2 ∗ √ d’Lambertian is written as = D D = ∇ − µ∂t , where D = ∇ − µ∂t. Unlike Baylis, which uses a “paravector” approach extensively for his relativistic treatment, this book ends with a relativistic treatment using STA. ENERGYMOMENTUMTENSORFORVECTORPARAMETERS. E

Did you cry cheater because of the reliance on brute force computer assisted symbolic algebra to ﬁnd the T(a) relations of eq. (3.116)? Or did you try this as a problem, and need some assistance? If so, here is an expansion of the energy momentum tensor for vector parameters. We start with

Fei = (E + IηH) ei (E.1) = Ei + E ∧ ei + Iη (Hi + H ∧ ei) .

To show that the scalar grades are related to the Poynting vector as hT(ei)i = −S · ei/c, we need the scalar grades of the tensor for vector parameters

D †E D ¨ E FeiF = ¨EiE + Iη (H ∧ ei) E + (E∧ei) · E + IηHiE 2 2 (((( + η −EiIH + (η ((H(∧ ei) · H − (E ∧ ei) IH + ηHiH 2 (E.2) D E = I2η (H × e ) E − η (E × e ) I2H 2 i i = − (E × H) · ei/c, which is the Poynting relationship that was asserted. For the vector grades we have

D †E FeiF = h(Ei + Iη (H ∧ ei) + E ∧ ei + IηHi)(E − IηH)i1 1 ( ((( = EiE + (Iη((H ∧ ei) E + (E ∧ ei) · E + IηHiE 1 D E + η −E IH + η (H ∧ e ) · H − (E∧e ) IH + ηH H (E.3) i i i i 1 2 2 2 2 2 = EiE + EEi − E ei + η HHi − η H ei + η HiH 2 2 2 = 2EiE − E ei + η 2HiH − H ei .

Assembling all the results, we have hT(e )i · e = 2E E − E2δ + η2 2H H − H2δ , (E.4) i 1 j 2 i j i j i j i j

i j which proves that hT(ei)i1 · e j = −Θ as stated in deﬁnition 3.5.

229

MATHEMATICANOTEBOOKS. F

These Mathematica notebooks, some just trivial ones used to generate ﬁgures, others more elaborate, and perhaps some even polished, can be found in https://github.com/peeterjoot/mathematica/tree/master/. The free Wolfram CDF player, is capable of read-only viewing these notebooks to some extent.

• Dec 18, 2016 GAelectrodynamics/projectionAndRejectionDiagram.nb Figure illustrating projection and rejection.

• Dec 19, 2016 GAelectrodynamics/oneParameterDifferentialFig.nb One parameter differential figure.

• Dec 20, 2016 GAelectrodynamics/twoParameterDifferentialFig.nb Two parameter differential figure.

• Sep 26, 2017 GAelectrodynamics/parallelograms.nb Overlapping parallelograms with ﬁxed areas. Figure: parrallelogramsFig1.eps.

• Sep 26, 2017 GAelectrodynamics/parallelogram.nb This is the notebook for two rotation ﬁgures. One is for a rotation of a vector lying in a plane (but that plane is viewed from a 3D vantage point), and the other is for a rotation with respect to a plane through an angle, and applied to a vector out of the plane.

• Oct 23, 2017 GAelectrodynamics/circularLineChargeDensity.nb Some messy evaluation of integrals that end up expressed in terms of elliptic E() and F() functions. Was associated with the evaluation of the charge of a circular segment of line charge.

• Oct 23, 2017 GAelectrodynamics/LineChargeIntegralsAndFigure.nb Integrals for Line charge problem, including some of the special angle cases that seem to require separate evaluation. Also has a plot linechargeFig1.eps, and some plots (not in the book) of the integrands.

231 232 mathematica notebooks.

• Nov 2, 2017 GAelectrodynamics/lineChargeArcFigure.nb Figure for circular arc of line charge. One arc of charge on the x-y plane at a ﬁxed radius. Field point, azimuthal angles for the range of the line charge.

• Nov 19, 2017 GAelectrodynamics/zcapPotential.nb Figure for (magnetic) vector potential: vectorPotentialFig1.eps.

• Nov 19, 2017 GAelectrodynamics/gaToroid.nb Cool toroidal segment ﬁgure for the book. toroidFig1.eps

• Nov 19, 2017 GAelectrodynamics/pillboxIntegrationVolumeFig1.nb This is the ﬁgure for pillbox integration volume that was used in the boundary value analysis of Maxwell’s equations.

• Nov 23, 2017 GAelectrodynamics/circularBasisCoordinatesInTermsOfJonesVector.nb Verify hand calculation from polarization.tex (also set as a problem). Got my hand calculation wrong. Try this with Mathematica instead. Has some additional checking of the solution.

• Nov 23, 2017 GAelectrodynamics/ellipticalPolarizationFig1.nb A plot of a rotated ellipse showing the major and minor axes, and the angle of rotation. This was related to an elliptically polarized plane wave.

• Nov 23, 2017 GAelectrodynamics/linearPolarizationFig1.nb Figure (linearPolarizationFig1.eps) showing the electric and magnetic field directions for a linearly polarized field propagating at a fixed angle to the horizontal in the transverse plane.

• Nov 24, 2017 GAelectrodynamics/pseudoscalarPolarizedRelationtoJones.nb Jones vector related calculations for GA representation of plane wave.

• Nov 28, 2017 GAelectrodynamics/vectorOrientationAndAdditionFigures.nb Vector addition and vector (and scalar) sign ﬁgures: VectorsWithOppositeOrientation- Fig1.eps, vectorAdditionFig1.eps, scalarOrientationFig1.eps.

• Dec 3, 2017 GAelectrodynamics/ellipticalPolarizationEnergyMomentumSimpliﬁcation.nb Hyperbolic cosine and arctan double angle reductions. Probably for cosh parameterization of an ellipse. mathematica notebooks. 233

• Dec 3, 2017 GAelectrodynamics/amperesLawMultiplePoints.nb Figure for amperesLawBetweenTwoCurrents.eps. Circles surrounding two currents, with respective phicap vectors around those sources.

• Dec 5, 2017 GAelectrodynamics/stressEnergyTensorValues.nb Uses my GA30.m package to compute the values of the energy momentum tensor multivectors, and relate those to the conventional tensor description of the same. Calculates the expansion of the adjoint of the energy momentum tensor, and also the expansion of some of the adjoint energy momentum tensor terms for the Poynting vector.

• Dec 13, 2017 GAelectrodynamics/planeCurrentIntegrals.nb Simple integrals for plane current distributions.

• Dec 14, 2017 GAelectrodynamics/ringIntegral2.nb Elliptic integrals for charge and current distribution on a ring.

• Dec 14, 2017 GAelectrodynamics/currentRingIntegrals.nb Some integrals related to circular current/charge distributions. A Manipulate that plots the magnitude of one of the integrands. A plot (chargeAndCurrentOnRingFig1.eps) that shows the geometric of the current ring and coordinate system used to solve or express the problem.

• Dec 17, 2017 GAelectrodynamics/cylinderFieldIntegrals.nb Symbolic evaluation of integrals for a cylindrical field distribution of finite and infinite length.

• Dec 17, 2017 GAelectrodynamics/ringFieldEllipticIntegralEquivalents.nb This notebook has transformation techniques to translate a couple of circular charge distribution integrals into their elliptic integral form. It also has plots of some of the electric and magnetic ﬁelds obtained from solving one such problem.

• Jan 24, 2018 GAelectrodynamics/stressTensorSymmetricDemo.nb A CliﬀordBasic calculation of the strain portion of the stress tensor, and an explicit demonstration that it is symmetric.

• Jan 28, 2018 GAelectrodynamics/exponentialFormOfVectorProductInR3.nb A somewhat random seeming complex exponential evaluation using CliﬀordBasic, and an R3 bivector argument. 234 mathematica notebooks.

• Jan 28, 2018 GAelectrodynamics/exponentialFormOfVectorProductInR2.nb Some R2 complex exponential calculations using CliﬀordBasic.

• Jan 28, 2018 GAelectrodynamics/compositionOfExponentials.nb This is a figure that has an equilateral triangle in the corner of the first quadrant. This was used to illustrate that the product of two complex exponentials is another complex exponential (in R3), but the bivector argument for that resulting exponential describes (in general) a different plane.

• Jan 29, 2018 GAelectrodynamics/radialVectorCylindricalFig1.nb Figure: radialVectorCylindricalFig1.eps. Notebook uses a dynamic (Manipulate) to generate the ﬁgure at a desirable angle and radius.

• Feb 1, 2018 GAelectrodynamics/dualityInR3Fig1.nb Figure (dualityInR3Fig1.eps) showing the R3 dual plane to a vector graphically. The scaling of the dual plane was only for illustration purposes and did not match the length of the vector.

• Feb 3, 2018 GAelectrodynamics/factorizationProblemVeriﬁcation.nb Verify answers for normal factorization problem. 2.16

• Feb 3, 2018 GAelectrodynamics/bivectorFactorizationFigures.nb Figures that illustrate two rectangular factorizations of a bivector in R3.

• Feb 5, 2018 GAelectrodynamics/neighbourhoodFig1.nb A nice little figure illustrating an infinitesimal neighbourhood around a given point. This was used as a figure in the somewhat tedious verification of a Green’s function, done in one of the appendixes.

• Feb 14, 2018 GAelectrodynamics/FourierTransformMathematicaParamsExploration.nb The purpose of this notebook is to show (i.e. decode) the meaning visually of the various Mathematica FourierTransform FourierParameters options available. Shows all the conventions (modern physics, pure math, signal processing, classical physics).

• Feb 20, 2018 GAelectrodynamics/ellipticalContoursFigures.nb Hyperbolic parameterization of an ellipse, and contours for the associated curvilinear coordinates. ellipticalContoursFig1.eps, and ellipticalContoursFig1.eps ﬁgures. mathematica notebooks. 235

• Feb 22, 2018 GAelectrodynamics/2dmanifoldPlot.nb Figure: 2dmanifoldFig1.eps. CliﬀordBasic calculation of the basis elements above and the area element. Same calculation using my GA30.m package. Generation of mmacell text for the book showing the input and output cells for the CliﬀordBasic calculation.

• Feb 24, 2018 GAelectrodynamics/reciprocalBasicCalculationFromFigure.nb Reciprocal basis computation with conventional vector algebra. Same calculation using bivectors. Display the cells for the book latex.

• Feb 24, 2018 GAelectrodynamics/linearSystemR4.nb A CliﬀordBasic solution to an R4 linear system a x + b y = c, using wedge products to solve. Also includes mmacell output to embed the solution in the book as Mathematica input and output.

• Feb 24, 2018 GAelectrodynamics/reflectionFigureGAcalculation.nb CliffordBasic calculations for Figure 1.20 reflection (reflectionFig1.eps), but not the figure itself. Also has mmacell output for the input and output cells for this calculation.

• Feb 24, 2018 GAelectrodynamics/curvilinearPolarFig1.nb Plot (curvilinearPolarFig1.eps) that shows a 2d vector in polar coordinates, the radial vector, and the angle relative to the horizon.

• Feb 25, 2018 GAelectrodynamics/sphericalPolar.nb Spherical polar basis and volume element. Calcuation of the curvilinear basis elements done with conventional vector algebra, and CliﬀordBasic. Also includes mmacell output for the book.

• Feb 28, 2018 GAelectrodynamics/orientedAreas.nb Bivector square and parallelogram ﬁgures, Figures for 90 degree rotations. Figure for line intersection. Figure for vector addition, showing scaled multiples of orthonormal bases elements.

• Feb 28, 2018 GAelectrodynamics/unitBivectorsFig.nb Unit bivectors ﬁgures in R3. unitBivectorsFig1.eps, unitBivectorsFig2.eps.

• Feb 28, 2018 GAelectrodynamics/unitBivectorAreaRepresentationsFig.nb A ﬁgure that shows diﬀerent shape representations of unit bivectors in R2. Includes parallelogram, square, circle and ellipse representations. Also includes inscribed arc to show the orientation of the bivectors. That was done using Arrow in combination with BSplineCurve, where the points on the curve come from evaluating CirclePoints. 236 mathematica notebooks.

• Feb 28, 2018 GAelectrodynamics/circularBivectorsIn3DFig1.nb This is the notebook for a few bivector related illustrations. The first is two circular representations of a bivector viewed from a 3D vantage point. Another is a bivector addition figure, with two bivectors summed in 3D. That figure was confusing (but cool), and has been left out of the book. The last figure separates the space between those bivectors summed in the second figure showing the summands and the sum all distinct. The current draft of the book includes this figure, but it is still a bit confusing.

• Apr 2, 2018 GAelectrodynamics/polarizationCircular.nb A hand calculation seemed to show that I had the wrong expressions for alphaL, alphaR in my polarization notes. Here’s a check of the correction of those expressions INDEX

ei j, ei jk, ···, 14 differential form, 88, 93, 96, 103 , 121 dimension,3 ∝, 157 divergence theorem, 110 RN,2 dot product,3, 28, 42 0-vector,6 dual, 26 1-vector,6 2-vector,7 electric charge density, 129 3-vector, 10 electric current density, 129 energy density, 162 anticommutation, 17 energy flux, 162 antisymmetric sum, 56 energy momentum tensor, 163 area element, 96 Euclidean space,5 Euler’s formula, 21 basis,3 bivector,7 far field, 201 blade, 34 Fourier transform, 110 boundary values, 210 frequency domain, 111 fundamental theorem of geometric calculus, circular polarization, 186 91 colinear vectors wedge, 33 gauge transformation, 198 commutation, 16, 53 grade, 12, 34 complex exponential, 21 grade selection, 14, 28 complex imaginary, 18, 35 gradient complex plane, 150 spherical, 87 complex power, 178 Gradient of the coordinates., 83 conjugation, 53 Green’s function, 111, 115 convolution, 124 Helmholtz, 117 Cramer’s rule, 60 Laplacian, 118 cross product, 31 curvilinear coordinates, 73, 77, 80, 85 Helmholtz Green’s function, 117 delta function, 124 Helmholtz operator, 114 determinant Helmholtz’s theorem, 122 wedge product, 31

237 238 Index

Jones vector, 184, 190 polar, 83 reciprocal frame, 65, 72, 73 k-vector, 12 reﬂection, 57 rejection, 45 Laplacian, 124 reverse, 34 Green’s function, 118 right circular polarization, 186 left circular polarization, 186 rotation, 20, 55 length,4 line charge, 147, 152 scalar,6 linear combination,2 scalar selection, 42 linear dependence,2 span,3 linear independence,3 spherical coordinates, 85, 90, 152 linear system, 58 standard basis,5 Lorenz gauge, 199 subspace,3 symmetric sum, 56 magnetic charge density, 129 magnetic current density, 129 tangent space, 77 Mathematica, 231 time harmonic, 111 Maxwell stress tensor, 163 toroid, 88 Maxwell’s equation, 132 trivector, 10 momentum density, 162 multivector, 12 unit pseudoscalar, 15 multivector dot product, 37 unit vector,5 multivector space, 12 multivector wedge product, 43 vector,6 vector derivative, 79 normal,5 vector inverse, 49 vector product, 27 oriented volume element, 77 vector space,1 orthonormal,5 volume element, 77, 103 volume parameterization, 103 parallelogram, 53 plane wave, 184 wedge factorization, 50 polar coordinates, 80 wedge product, 28 polar representation, 30 linear solution, 58 polarization, 184 Poynting vector, 162 projection, 45 pseudoscalar, 15, 19, 20, 35

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