The Liouville Equation in Atmospheric Predictability
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An Introduction to Quantum Field Theory
AN INTRODUCTION TO QUANTUM FIELD THEORY By Dr M Dasgupta University of Manchester Lecture presented at the School for Experimental High Energy Physics Students Somerville College, Oxford, September 2009 - 1 - - 2 - Contents 0 Prologue....................................................................................................... 5 1 Introduction ................................................................................................ 6 1.1 Lagrangian formalism in classical mechanics......................................... 6 1.2 Quantum mechanics................................................................................... 8 1.3 The Schrödinger picture........................................................................... 10 1.4 The Heisenberg picture............................................................................ 11 1.5 The quantum mechanical harmonic oscillator ..................................... 12 Problems .............................................................................................................. 13 2 Classical Field Theory............................................................................. 14 2.1 From N-point mechanics to field theory ............................................... 14 2.2 Relativistic field theory ............................................................................ 15 2.3 Action for a scalar field ............................................................................ 15 2.4 Plane wave solution to the Klein-Gordon equation ........................... -
On the Time Evolution of Wavefunctions in Quantum Mechanics C
On the Time Evolution of Wavefunctions in Quantum Mechanics C. David Sherrill School of Chemistry and Biochemistry Georgia Institute of Technology October 1999 1 Introduction The purpose of these notes is to help you appreciate the connection between eigenfunctions of the Hamiltonian and classical normal modes, and to help you understand the time propagator. 2 The Classical Coupled Mass Problem Here we will review the results of the coupled mass problem, Example 1.8.6 from Shankar. This is an example from classical physics which nevertheless demonstrates some of the essential features of coupled degrees of freedom in quantum mechanical problems and a general approach for removing such coupling. The problem involves two objects of equal mass, connected to two different walls andalsotoeachotherbysprings.UsingF = ma and Hooke’s Law( F = −kx) for the springs, and denoting the displacements of the two masses as x1 and x2, it is straightforward to deduce equations for the acceleration (second derivative in time,x ¨1 andx ¨2): k k x −2 x x ¨1 = m 1 + m 2 (1) k k x x − 2 x . ¨2 = m 1 m 2 (2) The goal of the problem is to solve these second-order differential equations to obtain the functions x1(t)andx2(t) describing the motion of the two masses at any given time. Since they are second-order differential equations, we need two initial conditions for each variable, i.e., x1(0), x˙ 1(0),x2(0), andx ˙ 2(0). Our two differential equations are clearly coupled,since¨x1 depends not only on x1, but also on x2 (and likewise forx ¨2). -
The Cambridge Mathematical Journal and Its Descendants: the Linchpin of a Research Community in the Early and Mid-Victorian Age ✩
View metadata, citation and similar papers at core.ac.uk brought to you by CORE provided by Elsevier - Publisher Connector Historia Mathematica 31 (2004) 455–497 www.elsevier.com/locate/hm The Cambridge Mathematical Journal and its descendants: the linchpin of a research community in the early and mid-Victorian Age ✩ Tony Crilly ∗ Middlesex University Business School, Hendon, London NW4 4BT, UK Received 29 October 2002; revised 12 November 2003; accepted 8 March 2004 Abstract The Cambridge Mathematical Journal and its successors, the Cambridge and Dublin Mathematical Journal,and the Quarterly Journal of Pure and Applied Mathematics, were a vital link in the establishment of a research ethos in British mathematics in the period 1837–1870. From the beginning, the tension between academic objectives and economic viability shaped the often precarious existence of this line of communication between practitioners. Utilizing archival material, this paper presents episodes in the setting up and maintenance of these journals during their formative years. 2004 Elsevier Inc. All rights reserved. Résumé Dans la période 1837–1870, le Cambridge Mathematical Journal et les revues qui lui ont succédé, le Cambridge and Dublin Mathematical Journal et le Quarterly Journal of Pure and Applied Mathematics, ont joué un rôle essentiel pour promouvoir une culture de recherche dans les mathématiques britanniques. Dès le début, la tension entre les objectifs intellectuels et la rentabilité économique marqua l’existence, souvent précaire, de ce moyen de communication entre professionnels. Sur la base de documents d’archives, cet article présente les épisodes importants dans la création et l’existence de ces revues. 2004 Elsevier Inc. -
An S-Matrix for Massless Particles Arxiv:1911.06821V2 [Hep-Th]
An S-Matrix for Massless Particles Holmfridur Hannesdottir and Matthew D. Schwartz Department of Physics, Harvard University, Cambridge, MA 02138, USA Abstract The traditional S-matrix does not exist for theories with massless particles, such as quantum electrodynamics. The difficulty in isolating asymptotic states manifests itself as infrared divergences at each order in perturbation theory. Building on insights from the literature on coherent states and factorization, we construct an S-matrix that is free of singularities order-by-order in perturbation theory. Factorization guarantees that the asymptotic evolution in gauge theories is universal, i.e. independent of the hard process. Although the hard S-matrix element is computed between well-defined few particle Fock states, dressed/coherent states can be seen to form as intermediate states in the calculation of hard S-matrix elements. We present a framework for the perturbative calculation of hard S-matrix elements combining Lorentz-covariant Feyn- man rules for the dressed-state scattering with time-ordered perturbation theory for the asymptotic evolution. With hard cutoffs on the asymptotic Hamiltonian, the cancella- tion of divergences can be seen explicitly. In dimensional regularization, where the hard cutoffs are replaced by a renormalization scale, the contribution from the asymptotic evolution produces scaleless integrals that vanish. A number of illustrative examples are given in QED, QCD, and N = 4 super Yang-Mills theory. arXiv:1911.06821v2 [hep-th] 24 Aug 2020 Contents 1 Introduction1 2 The hard S-matrix6 2.1 SH and dressed states . .9 2.2 Computing observables using SH ........................... 11 2.3 Soft Wilson lines . 14 3 Computing the hard S-matrix 17 3.1 Asymptotic region Feynman rules . -
Advanced Quantum Mechanics
Advanced Quantum Mechanics Rajdeep Sensarma [email protected] Quantum Dynamics Lecture #9 Schrodinger and Heisenberg Picture Time Independent Hamiltonian Schrodinger Picture: A time evolving state in the Hilbert space with time independent operators iHtˆ i@t (t) = Hˆ (t) (t) = e− (0) | i | i | i | i i✏nt Eigenbasis of Hamiltonian: Hˆ n = ✏ n (t) = cn(t) n c (t)=c (0)e− n | i | i n n | i | i n X iHtˆ iHtˆ Operators and Expectation: A(t)= (t) Aˆ (t) = (0) e Aeˆ − (0) = (0) Aˆ(t) (0) h | | i h | | i h | | i Heisenberg Picture: A static initial state and time dependent operators iHtˆ iHtˆ Aˆ(t)=e Aeˆ − Schrodinger Picture Heisenberg Picture (0) (t) (0) (0) | i!| i | i!| i Equivalent description iHtˆ iHtˆ Aˆ Aˆ Aˆ Aˆ(t)=e Aeˆ − ! ! of a quantum system i@ (t) = Hˆ (t) i@ Aˆ(t)=[Aˆ(t), Hˆ ] t| i | i t Time Evolution and Propagator iHtˆ (t) = e− (0) Time Evolution Operator | i | i (x, t)= x (t) = x Uˆ(t) (0) = dx0 x Uˆ(t) x0 x0 (0) h | i h | | i h | | ih | i Z Propagator: Example : Free Particle The propagator satisfies and hence is often called the Green’s function Retarded and Advanced Propagator The following propagators are useful in different contexts Retarded or Causal Propagator: This propagates states forward in time for t > t’ Advanced or Anti-Causal Propagator: This propagates states backward in time for t < t’ Both the retarded and the advanced propagator satisfies the same diff. eqn., but with different boundary conditions Propagators in Frequency Space Energy Eigenbasis |n> The integral is ill defined due to oscillatory nature -
The Tangled Tale of Phase Space David D Nolte, Purdue University
Purdue University From the SelectedWorks of David D Nolte Spring 2010 The Tangled Tale of Phase Space David D Nolte, Purdue University Available at: https://works.bepress.com/ddnolte/2/ Preview of Chapter 6: DD Nolte, Galileo Unbound (Oxford, 2018) The tangled tale of phase space David D. Nolte feature Phase space has been called one of the most powerful inventions of modern science. But its historical origins are clouded in a tangle of independent discovery and misattributions that persist today. David Nolte is a professor of physics at Purdue University in West Lafayette, Indiana. Figure 1. Phase space , a ubiquitous concept in physics, is espe- cially relevant in chaos and nonlinear dynamics. Trajectories in phase space are often plotted not in time but in space—as rst- return maps that show how trajectories intersect a region of phase space. Here, such a rst-return map is simulated by a so- called iterative Lozi mapping, (x, y) (1 + y − x/2, −x). Each color represents the multiple intersections of a single trajectory starting from dierent initial conditions. Hamiltonian Mechanics is geometry in phase space. ern physics (gure 1). The historical origins have been further —Vladimir I. Arnold (1978) obscured by overly generous attribution. In virtually every textbook on dynamics, classical or statistical, the rst refer- Listen to a gathering of scientists in a hallway or a ence to phase space is placed rmly in the hands of the French coee house, and you are certain to hear someone mention mathematician Joseph Liouville, usually with a citation of the phase space. -
Chapter 6. Time Evolution in Quantum Mechanics
6. Time Evolution in Quantum Mechanics 6.1 Time-dependent Schrodinger¨ equation 6.1.1 Solutions to the Schr¨odinger equation 6.1.2 Unitary Evolution 6.2 Evolution of wave-packets 6.3 Evolution of operators and expectation values 6.3.1 Heisenberg Equation 6.3.2 Ehrenfest’s theorem 6.4 Fermi’s Golden Rule Until now we used quantum mechanics to predict properties of atoms and nuclei. Since we were interested mostly in the equilibrium states of nuclei and in their energies, we only needed to look at a time-independent description of quantum-mechanical systems. To describe dynamical processes, such as radiation decays, scattering and nuclear reactions, we need to study how quantum mechanical systems evolve in time. 6.1 Time-dependent Schro¨dinger equation When we first introduced quantum mechanics, we saw that the fourth postulate of QM states that: The evolution of a closed system is unitary (reversible). The evolution is given by the time-dependent Schrodinger¨ equation ∂ ψ iI | ) = ψ ∂t H| ) where is the Hamiltonian of the system (the energy operator) and I is the reduced Planck constant (I = h/H2π with h the Planck constant, allowing conversion from energy to frequency units). We will focus mainly on the Schr¨odinger equation to describe the evolution of a quantum-mechanical system. The statement that the evolution of a closed quantum system is unitary is however more general. It means that the state of a system at a later time t is given by ψ(t) = U(t) ψ(0) , where U(t) is a unitary operator. -
2.-Time-Evolution-Operator-11-28
2. TIME-EVOLUTION OPERATOR Dynamical processes in quantum mechanics are described by a Hamiltonian that depends on time. Naturally the question arises how do we deal with a time-dependent Hamiltonian? In principle, the time-dependent Schrödinger equation can be directly integrated choosing a basis set that spans the space of interest. Using a potential energy surface, one can propagate the system forward in small time-steps and follow the evolution of the complex amplitudes in the basis states. In practice even this is impossible for more than a handful of atoms, when you treat all degrees of freedom quantum mechanically. However, the mathematical complexity of solving the time-dependent Schrödinger equation for most molecular systems makes it impossible to obtain exact analytical solutions. We are thus forced to seek numerical solutions based on perturbation or approximation methods that will reduce the complexity. Among these methods, time-dependent perturbation theory is the most widely used approach for calculations in spectroscopy, relaxation, and other rate processes. In this section we will work on classifying approximation methods and work out the details of time-dependent perturbation theory. 2.1. Time-Evolution Operator Let’s start at the beginning by obtaining the equation of motion that describes the wavefunction and its time evolution through the time propagator. We are seeking equations of motion for quantum systems that are equivalent to Newton’s—or more accurately Hamilton’s—equations for classical systems. The question is, if we know the wavefunction at time t0 rt, 0 , how does it change with time? How do we determine rt, for some later time tt 0 ? We will use our intuition here, based largely on correspondence to classical mechanics). -
Unitary Time Evolution
Unitary time evolution Time evolution of quantum systems is always given by Unitary Transformations. If the state of a quantum system is ψ , then at a later time | i ψ Uˆ ψ . | i→ | i Exactly what this operator Uˆ is will depend on the particular system and the interactions that it undergoes. It does not, however, depend on the state ψ . This | i means that time evolution of quantum systems is linear. Because of this linearity, if a system is in state ψ or φ or any linear combination, the time evolution is| giveni | byi the same operator: (α ψ + β φ ) Uˆ(α ψ + β φ ) = αUˆ ψ + βUˆ φ . | i | i → | i | i | i | i – p. 1/25 The Schrödinger equation As we have seen, these unitary operators arise from the Schrodinger¨ equation d ψ /dt = iHˆ (t) ψ /~, | i − | i where Hˆ (t) = Hˆ †(t) is the Hamiltonian of the system. Because this is a linear equation, the time evolution must be a linear transformation. We can prove that this must be a unitary transformation very simply. – p. 2/25 Suppose ψ(t) = Uˆ(t) ψ(0) for some matrix Uˆ(t) (which we don’t yet assume| i to be| unitary).i Plugging this into the Schrödinger equation gives us: dUˆ(t) dUˆ †(t) = iHˆ (t)Uˆ(t)/~, = iUˆ †(t)Hˆ (t)/~. dt − dt At t = 0, Uˆ(0) = Iˆ, so Uˆ †(0)Uˆ(0) = Iˆ. We see that d 1 Uˆ †(t)Uˆ(t) = Uˆ †(t) iHˆ (t) iHˆ (t) Uˆ(t) = 0. dt ~ − So Uˆ †(t)Uˆ(t) = Iˆ at all times t, and Uˆ(t) must always be unitary. -
Siméon-Denis Poisson Mathematics in the Service of Science
S IMÉ ON-D E N I S P OISSON M ATHEMATICS I N T H E S ERVICE O F S CIENCE E XHIBITION AT THE MATHEMATICS LIBRARY U NIVE RSIT Y O F I L L I N O I S A T U RBANA - C HAMPAIGN A U G U S T 2014 Exhibition on display in the Mathematics Library of the University of Illinois at Urbana-Champaign 4 August to 14 August 2014 in association with the Poisson 2014 Conference and based on SIMEON-DENIS POISSON, LES MATHEMATIQUES AU SERVICE DE LA SCIENCE an exhibition at the Mathematics and Computer Science Research Library at the Université Pierre et Marie Curie in Paris (MIR at UPMC) 19 March to 19 June 2014 Cover Illustration: Portrait of Siméon-Denis Poisson by E. Marcellot, 1804 © Collections École Polytechnique Revised edition, February 2015 Siméon-Denis Poisson. Mathematics in the Service of Science—Exhibition at the Mathematics Library UIUC (2014) SIMÉON-DENIS POISSON (1781-1840) It is not too difficult to remember the important dates in Siméon-Denis Poisson’s life. He was seventeen in 1798 when he placed first on the entrance examination for the École Polytechnique, which the Revolution had created four years earlier. His subsequent career as a “teacher-scholar” spanned the years 1800-1840. His first publications appeared in the Journal de l’École Polytechnique in 1801, and he died in 1840. Assistant Professor at the École Polytechnique in 1802, he was named Professor in 1806, and then, in 1809, became a professor at the newly created Faculty of Sciences of the Université de Paris. -
Transcendental Numbers
INTRODUCTION TO TRANSCENDENTAL NUMBERS VO THANH HUAN Abstract. The study of transcendental numbers has developed into an enriching theory and constitutes an important part of mathematics. This report aims to give a quick overview about the theory of transcen- dental numbers and some of its recent developments. The main focus is on the proof that e is transcendental. The Hilbert's seventh problem will also be introduced. 1. Introduction Transcendental number theory is a branch of number theory that concerns about the transcendence and algebraicity of numbers. Dated back to the time of Euler or even earlier, it has developed into an enriching theory with many applications in mathematics, especially in the area of Diophantine equations. Whether there is any transcendental number is not an easy question to answer. The discovery of the first transcendental number by Liouville in 1851 sparked up an interest in the field and began a new era in the theory of transcendental number. In 1873, Charles Hermite succeeded in proving that e is transcendental. And within a decade, Lindemann established the tran- scendence of π in 1882, which led to the impossibility of the ancient Greek problem of squaring the circle. The theory has progressed significantly in recent years, with answer to the Hilbert's seventh problem and the discov- ery of a nontrivial lower bound for linear forms of logarithms of algebraic numbers. Although in 1874, the work of Georg Cantor demonstrated the ubiquity of transcendental numbers (which is quite surprising), finding one or proving existing numbers are transcendental may be extremely hard. In this report, we will focus on the proof that e is transcendental. -
Lecture 6: Time Evolution and the Schrödinger Equation
8.04: Quantum Mechanics Professor Allan Adams Massachusetts Institute of Technology 2013 February 26 Lecture 6 Time Evolution and the Schr¨odinger Equation Assigned Reading: E&R 3all, 51;3;4;6 Li. 25−8, 31−3 Ga. 2all6=4 Sh. 3, 4 The Schr¨odinger equation is a partial differential equation. For instance, if pˆ2 m!2xˆ2 Eˆ = + ; 2m 2 then the Schr¨odinger equation becomes @ 2 @2 m!2x2 i = − ~ + : ~ @t 2m @x2 2 Of course, Eˆ depends on the system, and the Schr¨odinger equation changes accordingly. To fully solve this for a given Eˆ, there are a few different methods available, and those are through brute force, extreme cleverness, and numerical calculation. An elegant way that helps in all cases though makes use of superposition. Suppose that at t = 0, our system is in a state of definite energy. This means that (x; 0; E) = φ(x; E); where Eφˆ (x; E) = E · φ(x; E): Evolving it in time means that @ i E = E · : ~ @t E Given the initial condition, this is easily solved to be (x; t; E) = e −i!tφ(x; E) through the de Broglie relation E = ~!: Note that p(x; t) = j (x; t; E)j2 = jφ(x; E)j2 ; 2 8.04: Lecture 6 so the time evolution disappears from the probability density! That is why wavefunctions corresponding to states of definite energy are also called stationary states. So are all systems in stationary states? Well, probabilities generally evolve in time, so that cannot be. Then are any systems in stationary states? Well, nothing is eternal, and like the plane wave, the stationary state is only an approximation.