Category:Bethe-Salpeter equations: Difference between revisions

The formalism of the Bethe-Salpeter equation (BSE) allows for calculating the polarizability with the electron-hole interaction and constitutes the state of the art for calculating absorption spectra in solids.

Theory

The Bethe-Salpeter equation

In the BSE, the excitation energies correspond to the eigenvalues ${\displaystyle {\omega }_{\lambda }}$ of the following linear problem

${\displaystyle \left(\begin{array}{cc}\mathbf{𝐀}& \mathbf{𝐁}\\ {\mathbf{𝐁}}^{*}& {\mathbf{𝐀}}^{*}\end{array}\right)\left(\begin{array}{l}{\mathbf{𝐗}}_{\lambda }\\ {\mathbf{𝐘}}_{\lambda }\end{array}\right)={\omega }_{\lambda }\left(\begin{array}{cc}\mathbf{𝟏}& \mathbf{𝟎}\\ \mathbf{𝟎}& -\mathbf{𝟏}\end{array}\right)\left(\begin{array}{l}{\mathbf{𝐗}}_{\lambda }\\ {\mathbf{𝐘}}_{\lambda }\end{array}\right).}$

The matrices ${\displaystyle A}$ and ${\displaystyle A^{*}}$ describe the resonant and anti-resonant transitions between the occupied ${\displaystyle v,v^{\prime }}$ and unoccupied ${\displaystyle c,c^{\prime }}$ states

${\displaystyle A_{vc}^{v^{\prime }{c}^{\prime }}=({\epsilon }_v-{\epsilon }_c){\delta }_{v{v}^{\prime }}{\delta }_{c{c}^{\prime }}+⟨c{v}^{\prime }|V|v{c}^{\prime }⟩-⟨c{v}^{\prime }|W|c^{\prime }v⟩.}$

The energies and orbitals of these states are usually obtained in a ${\displaystyle G_0{W}_0}$ calculation, but DFT and Hybrid functional calculations can be used as well. The electron-electron interaction and electron-hole interaction are described via the bare Coulomb ${\displaystyle V}$ and the screened potential ${\displaystyle W}$.

The coupling between resonant and anti-resonant terms is described via terms ${\displaystyle B}$ and ${\displaystyle B^{*}}$

${\displaystyle B_{vc}^{v^{\prime }{c}^{\prime }}=⟨v{v}^{\prime }|V|c{c}^{\prime }⟩-⟨v{v}^{\prime }|W|c^{\prime }c⟩.}$

Due to the presence of this coupling, the Bethe-Salpeter Hamiltonian is non-Hermitian.

The Tamm-Dancoff approximation

A common approximation to the BSE is the Tamm-Dancoff approximation (TDA), which neglects the coupling between resonant and anti-resonant terms, i.e., ${\displaystyle B}$ and ${\displaystyle B^{*}}$. Hence, the TDA reduces the BSE to a Hermitian problem

${\displaystyle A{X}_{\lambda }={\omega }_{\lambda }{X}_{\lambda }.}$

In reciprocal space, the matrix ${\displaystyle A}$ is written as

${\displaystyle A_{vc\mathbf{𝐤}}^{v^{\prime }{c}^{\prime }{\mathbf{𝐤}}^{\prime }}=({\epsilon }_v-{\epsilon }_c){\delta }_{v{v}^{\prime }}{\delta }_{c{c}^{\prime }}{\delta }_{{\mathbf{𝐤}\mathbf{𝐤}}^{\prime }}+\frac{2}{\mathrm{\Omega }}\sum _{\mathbf{𝐆}\ne 0}{\overline{V}}_{\mathbf{𝐆}}(\mathbf{𝐪})⟨c\mathbf{𝐤}|e^{i\mathbf{𝐆}\mathbf{𝐫}}|v\mathbf{𝐤}⟩⟨v^{\prime }{\mathbf{𝐤}}^{\prime }|e^{-i\mathbf{𝐆}\mathbf{𝐫}}|c^{\prime }{\mathbf{𝐤}}^{\prime }⟩-\frac{2}{\mathrm{\Omega }}\sum _{{\mathbf{𝐆},\mathbf{𝐆}}^{\prime }}{W}_{{\mathbf{𝐆},\mathbf{𝐆}}^{\prime }}(\mathbf{𝐪},\omega ){\delta }_{{\mathbf{𝐪},\mathbf{𝐤}\mathbf{-}\mathbf{𝐤}}^{\prime }}⟨c\mathbf{𝐤}|e^{i(\mathbf{𝐪}\mathbf{+}\mathbf{𝐆})}|c^{\prime }{\mathbf{𝐤}}^{\prime }⟩⟨v^{\prime }{\mathbf{𝐤}}^{\prime }|e^{-i(\mathbf{𝐪}\mathbf{+}\mathbf{𝐆})}|v\mathbf{𝐤}⟩,}$

where ${\displaystyle \mathrm{\Omega }}$ is the cell volume, ${\displaystyle \overline{V}}$ is the bare Coulomb potential without the long-range part

${\displaystyle {\overline{V}}_{\mathbf{𝐆}}(\mathbf{𝐪})=\{\begin{array}{ll}0& \text{ if }G=0\\ V_{\mathbf{𝐆}}(\mathbf{𝐪})=\frac{4\pi }{|\mathbf{𝐪}+\mathbf{𝐆}{|}^2}& \text{ else }\end{array},}$

and the screened Coulomb potential ${\displaystyle W_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}(\mathbf{𝐪},\omega )=\frac{4\pi {ϵ}_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}^{-1}(\mathbf{𝐪},\omega )}{|\mathbf{𝐪}+\mathbf{𝐆}||\mathbf{𝐪}+{\mathbf{𝐆}}^{\prime }|}.}$

Here, the dielectric function ${\displaystyle {ϵ}_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}(\mathbf{𝐪})}$ describes the screening in ${\displaystyle W}$ within the random-phase approximation (RPA)

${\displaystyle {ϵ}_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}^{-1}(\mathbf{𝐪},\omega )={\delta }_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}+\frac{4\pi }{|\mathbf{𝐪}+\mathbf{𝐆}{|}^2}{\chi }_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}^{\mathrm{R}\mathrm{P}\mathrm{A}}(\mathbf{𝐪},\omega ).}$

Although the dielectric function is frequency-dependent, the static approximation ${\displaystyle W_{\mathbf{𝐆},{\mathbf{𝐆}}^{\prime }}(\mathbf{𝐪},\omega =0)}$ is considered a standard for practical BSE calculations.

The macroscopic dielectric which account for the excitonic effects is found via eigenvalues ${\displaystyle {\omega }_{\lambda }}$ and eigenvectors ${\displaystyle X_{\lambda }}$ of the BSE

${\displaystyle {ϵ}_M(\mathbf{𝐪},\omega )=1+\underset{\mathbf{𝐪}\to 0}{\lim }v(q)\sum _{\lambda }{|\sum _{c,v,k}⟨c\mathbf{𝐤}|e^{i\mathbf{𝐪}\mathbf{𝐫}}|v\mathbf{𝐤}⟩X_{\lambda }^{cv\mathbf{𝐤}}|}^2\times (\frac{1}{{\omega }_{\lambda }-\omega -i\delta }+\frac{1}{{\omega }_{\lambda }+\omega +i\delta }).}$

Scaling

The scaling of the BSE equation strongly limits its application for large systems. The main limiting factor is the diagonalization of the BSE Hamiltonian. The rank of the Hamiltonian is

${\displaystyle N_{\mathrm{r}\mathrm{a}\mathrm{n}\mathrm{k}}=N_k\times N_c\times N_v}$,

where ${\displaystyle N_k}$ is the number of k-points in the Brillouin zone and ${\displaystyle N_c}$ and ${\displaystyle N_v}$ are the number of conduction and valence bands, respectively. The diagonalization of the matrix scales cubically with the matrix rank, i.e., ${\displaystyle N_{\mathrm{r}\mathrm{a}\mathrm{n}\mathrm{k}}^3}$.

Despite the fact that this matrix diagonalization is usually the bottleneck for bigger systems, the construction of the BSE Hamiltonian also scales unfavorably and can play a dominant role in big systems, i.e.,

${\displaystyle N_k\times N_q\times (N_v\times N_v\times N_G\times N_c\times N_c)}$,

where ${\displaystyle N_q}$ is the number of q-points and ${\displaystyle N_G}$ number of G-vectors.

How to

• BSE calculations

References