Quantum Mechanics, Volume 3. Claude Cohen-Tannoudji

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amounts to imposing the |φn〉 to be not only eigenvectors of , but also of the operator HHF defined by (74) in the entire one-particle state space (without the restriction to ); consequently, the |φn〉 must obey:

(77)

Operator HHF is defined in (74), where the operator WHF is given by (60) and depends on the projector PN. This last operator may be expressed as a function of the |φn〉 in the same way as with the |θi〉, and relation (48) may be replaced by:

(78)

Relations (77), together with definition (60) where (78) has been inserted, are a set of equations allowing the self-consistent determination of the |φn〉; they are called the Hartree-Fock equations. This operator form (77) is simpler than the one obtained in § 1-c; it emphasizes the similarity with the usual eigenvalue equation for a single particle moving in an external potential, illustrating the concept of a self-consistent mean field. One must keep in mind, however, that via the projector (78) included in WHF, this particle moves in a potential depending on the whole set of states occupied by all the particles. Remember also that we did not carry out an exact computation, but merely presented an approximate theory (variational method).

      The discussion in § 1-f is still relevant. As the operator WHF depends on the |φn〉, the Hartree-Fock equations have an intrinsic nonlinear character, which generally requires a resolution by successive approximations. We start from a set of N individual states to build a first value of PN and the operator WHF, which are used to compute the Hamiltonian (74). Considering this Hamiltonian now fixed, the Hartree-Fock equations (77) become linear, and can be solved as usual eigenvalue equations. This leads to new values for the |φn〉, and finishes the first iteration. In the second iteration, we use the in (78) to compute a new value of the mean field operator WHF; considering again this operator as fixed, we solve the eigenvalue equation and obtain the second iteration values for the |φn〉, and so on. If the initial values are physically reasonable, one can hope for a rapid convergence towards the expected solution of the nonlinear Hartree-Fock equations.

      The variational energy can be computed in the same way as in § 1-e. Multiplying on the left equation (77) by the bra 〈φn|, we get:

      (79)

      After summing over the subscript n, we obtain:

      (80)

Taking into account (51), (53), and (61), we get:

      (81)

      where the particle interaction energy is counted twice. To compute the energy , we can eliminate between (26) and this relation and we finally obtain:

      (82)

2-d. Hartree-Fock equations for electrons

      Assume the fermions we are studying are particles with spin 1/2, electrons for example. The basis {|r〉} of the individual states used in § 1 must be replaced by the basis formed with the kets {|r, ν)}, where ν is the spin index, which can take 2 distinct values noted ±1/2, or more simply ±. To the summation over d³r we must now add a summation over the 2 values of the index spin ν. A vector |φ〉 in the individual state space is now written:

      (83)

      with:

      (84)

      The variables r and ν play a similar role but the first one is continuous whereas the second is discrete. Writing them in the same parenthesis might hide this difference, and we often prefer noting the discrete index as a superscript of the function φ and write:

      (85)

Let us build an N particle variational state from N orthonormal states , with n =1, 2,.. , N. Each of the describes an individual state including the spin and position variables; the first N₊ values of νn (n = 1,2,..N₊) are equal to +1/2, the last N_– are equal to –1/2, with N₊ + N_– = N (we assume N₊ and N_- are fixed for the moment but we may allow them to vary later to enlarge the variational family). In the space of the individual states, we introduce a complete basis

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