Note: this page is under construction.
A full treatment of spin, along with its coupling to the orbital angular momentum, is given through the Dirac equation. The Schrodinger equation does not include spin. There is a compromise, however, namely to make a “scalar” approximation to the Dirac equation which removes coupling between orbital and spin parts. In this case the Dirac 4-vector becomes a pair of 2-vectors (large and small components). Most codes make a “scalar Dirac” approximation. The missing coupling can be added perturbatively. How good this approximation is can be checked against solutions of the full Dirac equation. Since the vast majority of this coupling originates from points very close to a nucleus where the electron velocity is large, it can be well approximated by considering the spherical part of the potential only. This results in a spin-orbit term of the form , where
is dominated by a small region near the nucleus where diverges in proportion to .
Additionally a magnetic field can be added to the potential. This can originate from a true external magnetic field, or from an “exchange-correlation” field which is in fact a coulomb field that acts in the same way as a magnetic field, as a consequence of the Pauli principle.1. This is the primary origin of magnetization in materials. If the spins are collinear, this can be parameterized in density-functional theory as . and are functionals of some combination of the charge and spin densities, i.e. and .
DFT codes typically compute magnetic phenomena by allowing spin densities to form (when the magnetic energy gain is strong enough to surmount the kinetic energy cost), resulting in different spin-up and spin-down potentials. Most of the time this is sufficient, in which case it is possible to treat spin phenomena as two independent cases, with independent “spin up” and “spin down” potentials. While potentials are uncoupled the two solutions do couple through the self-consistency cycle, as the (separately calculated) and evolve and modify .
It is possible to allow the spin quantization axis to vary in space. Then “up” and “down” have a local meaning that depend on the local spin quantization axis. When the spin quantization axis varies in space, and rotate also, and the effective one-particle equations couple. In that case the (scalar) Dirac equation becomes a 2×2 matrix in spin space.
When spin-orbit coupling is taken into account, it has a contribution proportional to , which adds to the up- and down- parts of the effective single-particle potential. This term does not couple the two channels. There are additionally terms and which couple up- and down- parts. Thus, even when the spin-quantization axis is assumed to be collinear, coupling between the up and down potential subsists through these terems, and the scalar Dirac equation becomes a 2×2 matrix in spin space through . This coupling also can modify the spin quantization axis in an r-dependent way. Typically (but not always) the noncollinearity induced by modifies the energy only slightly, and it is sufficient to restrict the input potential to a collinear one.
Magnetism in the full potential code lmf
lmf has a limited ability to handle noncollinearity, but it is not (as of this writing) a fully noncollinear implementation. The input potential can be magnetic and spin-orbit coupling can be included, but the noncollinear parts of the output density are discarded so that the input potential is always collinear. (Note that in the absence of magnetism, this is not an approximation).
Spin-Orbit coupling in lmf
Spin-orbit coupling can be treated at varying levels of approximation, through token SO in HAM.
SO=1 adds the standard spin-orbit coupling, . to the one-body hamiltonian. For each site matrix elements are calculated and added to the augmented part of the hamiltonian. The various contributions to this is a one-body term are also added to the total energy.
Further, information about SO coupling can be resolved by site.
SO=2 adds only the diagonal part, . This preserves the independence of the spin channels. It is, however, an approximation.
SO=3 initially adds only the to the hamiltonian, preserving the independence of the spin channels in the eigenvectors. The eigenvectors are the same as for SO=2. However, the off-diagonal parts and are included in perturbation theory, to modify the eigenvalues but not eigenvectors. This approximation is reasonable since the total energy is variational in the density, so it does not need to be as accurately described as the eigenvalues. The perturbation theory is a bit different from standard, as it avoids difficulties when two states are nearly degenerate. See the Appendix in Phys. Rev. B89, 155204.
This is a much improved approximation to SO=1, while staying within a collinear framework.
Magnetism in the GW code
The GW code can handle magnetic systems. Here the magnetism originates from the exact exchange; it is generally much superior to LDA-based magnetic calculations.
The GW code cannot handle noncollinear eigenvectors as yet
, so you must run one-shot GW or QS_GW_ without SO coupling, or include in the SO=2 or SO=3 approximations. Apart from very special cases,
In some cases, e.g. CoO, time-reversal symmetry can be broken. In that case
Spin orbit coupling used in conjunction with QSGW
Magnetism in the ASA code lm
Magnetism in the ASA code Green’s function codes lmgf and lmpg
Magnetism in the tight-binding code tbe
… To be written
1 R. M. Martin, Electronic Structure, Cambridge University Press (2004).
2 Federico Brivio, Keith T. Butler, Aron Walsh, and Mark van Schilfgaarde, “Relativistic quasiparticle self-consistent electronic structure of hybrid halide perovskite photovoltaic absorbers,” Phys. Rev B89, 155204 (2014)