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Introduction to Electronic Structure Theory 1 Introduction 2 What Is Introduction to Electronic Structure Theory C. David Sherrill School of Chemistry and Biochemistry Georgia Institute of Technology June 2002 Last Revised: June 2003 1 Introduction The purpose of these notes is to give a brief introduction to electronic structure theory and to introduce some of the commonly used notation. Chapters 1-2 of Szabo and Ostlund [1] are highly recommended for this topic. 2 What is Electronic Structure Theory? Electronic Structure Theory describes the motions of electrons in atoms or molecules. Generally this is done in the context of the Born-Oppenheimer Approximation, which says that electrons are so much lighter (and therefore faster) than nuclei that they will ¯nd their optimal distribution for any given nuclear con¯guration. The electronic energy at each nuclear con¯guration is the potential energy that the nuclei feel, so solving the electronic problem for a range of nuclear con¯gurations gives the potential energy surface. Because the electrons are so small, one needs to use quantum mechanics to solve for their motion. Quantum mechanics tells us that the electrons will not be localized at particular points in space, but they are best thought of as \matter waves" which can interfere. The probability of ¯nding a single electron at a given point in space is given by ª¤(x)ª(x) for its wavefunction ª at the point x. The wavefunction can be determined by solving the time-independent SchrÄodinger equation H^ ª = Eª. If the problem is time-dependent, then the time-dependent SchrÄodinger @ª ^ equation {h¹ @t = Hª must be used instead; otherwise, the solutions to the time-independent problem are also solutions to the time-dependent problem when they are multiplied by the energy dependent phase factor e¡iEt=h¹ . Since we have ¯xed the nuclei under the Born-Oppenheimer approximation, we solve for the nonrelativistic electronic SchrÄodinger equation: 2 2 2 2 2 ^ h¹ 2 h¹ 2 ZAe ZAZBe e H = i A + + ; (1) ¡2m Xi r ¡ XA 2MA r ¡ XA;i 4¼²0rAi A>BX 4¼²0RAB Xi>j 4¼²0rij 1 where i; j refer to electrons and A; B refer to nuclei. In atomic units, this simpli¯es to: ^ 1 2 1 2 ZA ZAZB 1 H = i A + + : (2) ¡2 Xi r ¡ XA 2MA r ¡ XA;i rAi A>BX RAB Xi>j rij This Hamiltonian is appropriate as long as relativistic e®ects are not important for the system in question. Roughly speaking, relativistic e®ects are not generally considered important for atoms with atomic number below about 25 (Mn). For heavier atoms, the inner electrons are held more tightly to the nucleus and have velocities which increase as the atomic number increases; as these velocities approach the speed of light, relativistic e®ects become more important. There are various approaches for accounting for relativistic e®ects, but the most popular is to use relativistic e®ective core potentials (RECPs), often along with the standard nonrelativistic Hamiltonian above. 3 Properties Predicted by Electronic Structure Theory According to one of the postulates of quantum mechanics (see below), if we know the wavefunction ª(r; t) for a given system, then we can determine any property of that system, at least in principle. Obviously if we use approximations in determining the wavefunction, then the properties obtained from that wavefunction will also be approximate. Since we almost always invoke the Born-Oppenheimer approximation, we only have the elec- tronic wavefunction, not the full wavefunction for electrons and nuclei. Therefore, some properties involving nuclear motion are not necessarily available in the context of electronic structure theory. To fully understand the details of a chemical reaction, we need to use the electronic structure results to carry out subsequent dynamics computations. Fortunately, however, quite a few prop- erties are within the reach of just the electronic problem. For example, since the electronic energy is the potential energy felt by the nuclei, minimizing the electronic energy with respect to nuclear coordinates gives an equilibrium con¯guration of the molecule (which may be the global or just a local minimum). The electronic wavefunction or its various derivatives are su±cient to determine the following properties: Geometrical structures (rotational spectra) ² Rovibrational energy levels (infrared and Raman spectra) ² Electronic energy levels (UV and visible spectra) ² Quantum Mechanics + Statistical Mechanics Thermochemistry (¢H, ¢S, ¢G, Cv, Cp), ² primarily gas phase. ! 2 Potential energy surfaces (barrier heights, transition states); with a treatment of dynamics, ² this leads to reaction rates and mechanisms. Ionization potentials (photoelectron and X-ray spectra) ² Electron a±nities ² Franck-Condon factors (transition probabilities, vibronic intensities) ² IR and Raman intensities ² Dipole moments ² Polarizabilities ² Electron density maps and population analyses ² Magnetic shielding tensors NMR spectra ² ! 4 Postulates of Quantum Mechanics 1. The state of a quantum mechanical system is completely speci¯ed by the wavefunction ª(r; t). 2. To every observable in classical mechanics, there corresponds a linear, Hermitian opera- tor in quantum mechanics. For example, in coordinate space, the momentum operator P^x corresponding to momentum p in the x direction for a single particle is ih¹ @ . x ¡ @x 3. In any measurement of the observable associated with operator A^, the only values that will ever be observed are the eigenvalues a which satisfy A^ª = aª. Although measurements must always yield an eigenvalue, the state does not originally have to be in an eigenstate of A^. An arbitrary state can be expanded in the complete set of eigenvectors of A^ (AÃ^ i = aiÃi) as ª = i ciÃi, where the sum can run to in¯nity in principle. The probability of observing P ¤ eigenvalue ai is given by ci ci. 4. The average value of the observable corresponding to operator A^ is given by 1 ¤ ^ ¡1 ª Aªd¿ A = R 1 ¤ : (3) h i ¡1 ª ªd¿ R 5. The wavefunction evolves in time according to the time-dependent SchrÄodinger equation @ª H^ ª(r; t) = ih¹ (4) @t 3 6. The total wavefunction must be antisymmetric with respect to the interchange of all coor- dinates of one fermion with those of another. Electronic spin must be included in this set of coordinates. The Pauli exclusion principle is a direct result of this antisymmetry principle. 5 Dirac Notation For the purposes of solving the electronic SchrÄodinger equation on a computer, it is very convenient to turn everything into linear algebra. We can represent the wavefunctions ª(r) as vectors: n ª = ai ª^ i ; (5) j i Xi=1 j i where ª is called a \state vector," a are the expansion coe±cients (which may be complex), j i i and ª^ i are ¯xed \basis" vectors. A suitable (in¯nite-dimensional) linear vector space for such decompj iositions is called a \Hilbert space." We can write the set of coe±cients a as a column vector, f ig a1 0 a2 1 ª = B . C : (6) j i B . C B C B C @ an A In Dirac's \bracket" (or bra-ket) notation, we call ª a \ket." What about the adjoint of this vector? It is a row vector denoted by ª , which is calledj i a \bra" (to spell \bra-ket"), h j ¤ ¤ ¤ ª = (a1a2 a ): (7) h j ¢ ¢ ¢ n In linear algebra, the scalar product (ªa; ªb) between two vectors ªa and ªb is just b1 0 2 1 n ¤ ¤ ¤ b ¤ (ªa; ªb) = (a1a2 an) B . C = ai bi; (8) ¢ ¢ ¢ B . C X=1 B C i B C @ bn A assuming the two vectors are represented in the same basis set and that the basis vectors are orthonormal (otherwise, overlaps between the basis vectors, i.e., the \metric," must be included). The quantum mechanical shorthand for the above scalar product in bra-ket notation is just n ¤ ªa ªb = ai bi: (9) h j i Xi=1 4 Frequently, one only writes the subscripts a and b in the Dirac notation, so that the above dot product might be referred to as just a b . The order of the vectors ªa and ªb in a dot product h j i ¤ matters if the vectors can have complex numbers for their components, since (ªa; ªb) = (ªb; ªa) . Now suppose that we want our basis set to be every possible value of coordinate x. Apart from giving us a continuous (and in¯nite) basis set, there is no formal di±culty with this. We can then represent an arbitrary state as: 1 ª = ax x dx: (10) j i Z¡1 j i What are the coe±cients ax? It turns out that these coe±cients are simply the value of the wavefunction at each point x. That is, 1 ª = ª(x) x dx: (11) j i Z¡1 j i Since any two x coordinates are considered orthogonal (and their overlap gives a Dirac delta function), the scalar product of two state functions in coordinate space becomes 1 ¤ ªa ªb = ªa(x)ªb(x)dx: (12) h j i Z¡1 Now we turn our attention to matrix representations of operators. An operator A^ can be characterized by its e®ect on the basis vectors. The action of A^ on a basis vector ª^ j yields some 0 j i new vector ªj which can be expanded in terms of the basis vectors so long as we have a complete basis set. j i n ^ ^ 0 ^ A ªj = ªj = ªi Aij (13) j i j i Xi j i If we know the e®ect of A^ on the basis vectors, then we know the e®ect of A^ on any arbitrary vector because of the linearity of A^.
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