Gross–Pitaevskii equation

The Gross–Pitaevskii equation (GPE, named after Eugene P. Gross ^[1] and Lev Petrovich Pitaevskii ^[2]) describes the ground state of a quantum system of identical bosons using the Hartree–Fock approximation and the pseudopotential interaction model.

In the Hartree–Fock approximation the total wave-function $\Psi$ of the system of $N$ bosons is taken as a product of single-particle functions $\psi$,

$\Psi ({\mathbf {r}}_{1},{\mathbf {r}}_{2},\dots ,{\mathbf {r}}_{N})=\psi ({\mathbf {r}}_{1})\psi ({\mathbf {r}}_{2})\dots \psi ({\mathbf {r}}_{N})$

where $\mathbf {r} _{i}$ is the coordinate of the $i$-th boson.

The pseudopotential model Hamiltonian of the system is given as

$H=\sum _{{i=1}}^{N}\left(-{\hbar ^{2} \over 2m}{\partial ^{2} \over \partial {\mathbf {r}}_{i}^{2}}+V({\mathbf {r}}_{i})\right)+\sum _{{i<j}}{4\pi \hbar ^{2}a_{s} \over m}\delta ({\mathbf {r}}_{i}-{\mathbf {r}}_{j}),$

where $m$ is the mass of the boson, $V$ is the external potential, $a_{s}$ is the boson-boson scattering length, and $\delta ({\mathbf {r}})$ is the Dirac delta-function.

If the single-particle wave-function satisfies the Gross–Pitaevski equation,

$\left(-{\frac {\hbar ^{2}}{2m}}{\partial ^{2} \over \partial {\mathbf {r}}^{2}}+V({\mathbf {r}})+{4\pi \hbar ^{2}a_{s} \over m}\vert \psi ({\mathbf {r}})\vert ^{2}\right)\psi ({\mathbf {r}})=\mu \psi ({\mathbf {r}}),$

the total wave-function minimizes the expectation value of the model Hamiltonian under normalization condition $\int dV |\Psi|^2=N.$

It is a model equation for the single-particle wavefunction in a Bose–Einstein condensate. It is similar in form to the Ginzburg–Landau equation and is sometimes referred to as a nonlinear Schrödinger equation.

A Bose–Einstein condensate (BEC) is a gas of bosons that are in the same quantum state, and thus can be described by the same wavefunction. A free quantum particle is described by a single-particle Schrödinger equation. Interaction between particles in a real gas is taken into account by a pertinent many-body Schrödinger equation. If the average spacing between the particles in a gas is greater than the scattering length (that is, in the so-called dilute limit), then one can approximate the true interaction potential that features in this equation by a pseudopotential. The non-linearity of the Gross–Pitaevskii equation has its origin in the interaction between the particles. This is made evident by setting the coupling constant of interaction in the Gross–Pitaevskii equation to zero (see the following section): thereby, the single-particle Schrödinger equation describing a particle inside a trapping potential is recovered.

Form of equation

The equation has the form of the Schrödinger equation with the addition of an interaction term. The coupling constant, g, is proportional to the scattering length $a_{s}$ of two interacting bosons:

$g={\frac {4\pi \hbar ^{2}a_{s}}{m}}$,

where $\hbar$ is the reduced Planck's constant and m is the mass of the boson. The energy density is

${\mathcal {E}}={\frac {\hbar ^{2}}{2m}}\vert \nabla \Psi ({\mathbf {r}})\vert ^{2}+V({\mathbf {r}})\vert \Psi ({\mathbf {r}})\vert ^{2}+{\frac {1}{2}}g\vert \Psi ({\mathbf {r}})\vert ^{4},$

where $\Psi$ is the wavefunction, or order parameter, and V is an external potential. The time-independent Gross–Pitaevskii equation, for a conserved number of particles, is

$\mu \Psi ({\mathbf {r}})=\left(-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}+V({\mathbf {r}})+g\vert \Psi ({\mathbf {r}})\vert ^{2}\right)\Psi ({\mathbf {r}})$

where $\mu$ is the chemical potential. The chemical potential is found from the condition that the number of particles is related to the wavefunction by

$N=\int \vert \Psi ({\mathbf {r}})\vert ^{2}\,d^{3}r.$

From the time-independent Gross–Pitaevskii equation, we can find the structure of a Bose–Einstein condensate in various external potentials (e.g. a harmonic trap).

The time-dependent Gross–Pitaevskii equation is

$i\hbar {\frac {\partial \Psi ({\mathbf {r}},t)}{\partial t}}=\left(-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}+V({\mathbf {r}})+g\vert \Psi ({\mathbf {r}},t)\vert ^{2}\right)\Psi ({\mathbf {r}},t).$

From the time-dependent Gross–Pitaevskii equation we can look at the dynamics of the Bose–Einstein condensate. It is used to find the collective modes of a trapped gas.

Solutions

Since the Gross–Pitaevskii equation is a nonlinear, partial differential equation, exact solutions are hard to come by. As a result, solutions have to be approximated via myriad techniques.

Exact solutions

Free particle

The simplest exact solution is the free particle solution, with $V({\mathbf {r}})=0$,

$\Psi ({\mathbf {r}})={\sqrt {{\frac {N}{V}}}}e^{{i{\mathbf {k}}\cdot {\mathbf {r}}}}.$

This solution is often called the Hartree solution. Although it does satisfy the Gross–Pitaevskii equation, it leaves a gap in the energy spectrum due to the interaction:

$E({\mathbf {k}})=N\left[{\frac {\hbar ^{2}k^{2}}{2m}}+g{\frac {N}{2V}}\right].$

According to the Hugenholtz–Pines theorem, ^[3] an interacting bose gas does not exhibit an energy gap (in the case of repulsive interactions).

Soliton

A one-dimensional soliton can form in a Bose–Einstein condensate, and depending upon whether the interaction is attractive or repulsive, there is either a bright or dark soliton. Both solitons are local disturbances in a condensate with a uniform background density.

If the BEC is repulsive, so that $g>0$, then a possible solution of the Gross–Pitaevskii equation is,

$\psi (x)=\psi _{0}\tanh \left({\frac {x}{{\sqrt {2}}\xi }}\right)$,

where $\psi _{0}$ is the value of the condensate wavefunction at $\infty$, and $\xi =\hbar /{\sqrt {2mn_{0}g}}$, is the coherence length. This solution represents the dark soliton, since there is a deficit of condensate in a space of nonzero density. The dark soliton is also a type of topological defect, since $\psi$ flips between positive and negative values across the origin, corresponding to a $\pi$ phase shift.

For $g<0$

$\psi (x,t)=\psi (0)e^{{-i\mu t/\hbar }}{\frac {1}{\cosh \left[{\sqrt {2m\vert \mu \vert /\hbar ^{2}}}x\right]}},$

where the chemical potential is $\mu =g\vert \psi (0)\vert ^{2}/2$. This solution represents the bright soliton, since there is a concentration of condensate in a space of zero density.

Variational solutions

In systems where an exact analytical solution may not be feasible, one can make a variational approximation. The basic idea is to make a variational ansatz for the wavefunction with free parameters, plug it into the free energy, and minimize the energy with respect to the free parameters.

Thomas–Fermi approximation

If the number of particles in a gas is very large, the interatomic interaction becomes large so that the kinetic energy term can be neglected from the Gross–Pitaevskii equation. This is called the Thomas–Fermi approximation.

$\psi (x,t)={\sqrt {{\frac {\mu -V(x)}{NU_{0}}}}}$

Bogoliubov approximation

Bogoliubov treatment of the Gross–Pitaevskii equation is a method that finds the elementary excitations of a Bose–Einstein condensate. To that purpose, the condensate wavefunction is approximated by a sum of the equilibrium wavefunction $\psi _{0}={\sqrt {n}}e^{{-i\mu t}}$ and a small perturbation $\delta \psi$,

$\psi =\psi _{0}+\delta \psi$.

Then this form is inserted in the time dependent Gross–Pitaevskii equation and its complex conjugate, and linearized to first order in $\delta \psi$

$-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}\delta \psi +V\delta \psi +g(2|\psi _{0}|^{2}\delta \psi +\psi ^{2}\delta \psi ^{*})=i\hbar {\frac {\partial \delta \psi }{\partial t}}$

$-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}\delta \psi ^{*}+V\delta \psi ^{*}+g(2|\psi _{0}|^{2}\delta \psi ^{*}+(\psi ^{*})^{2}\delta \psi )=-i\hbar {\frac {\partial \delta \psi ^{*}}{\partial t}}$

Assuming the following for $\delta \psi$

${\displaystyle \delta \psi =e^{-i\mu t/\hbar }(u({\boldsymbol {r}})e^{-i\omega t}-v^{*}({\boldsymbol {r}})e^{i\omega t})}$

one finds the following coupled differential equations for $u$ and $v$ by taking the $e^{{\pm i\omega t}}$ parts as independent components

${\displaystyle \left(-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}+V+2gn-\hbar \mu -\hbar \omega \right)u-gnv=0}$

${\displaystyle \left(-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}+V+2gn-\hbar \mu +\hbar \omega \right)v-gnu=0}$

For a homogeneous system, i.e. for $V({\boldsymbol {r}})=const.$, one can get $V=\hbar \mu -gn$ from the zeroth order equation. Then we assume $u$ and $v$ to be plane waves of momentum ${\boldsymbol {q}}$, which leads to the energy spectrum

$\hbar \omega =\epsilon _{{\boldsymbol {q}}}={\sqrt {{\frac {\hbar ^{2}{\boldsymbol {q}}^{2}}{2m}}\left({\frac {\hbar ^{2}{\boldsymbol {q}}^{2}}{2m}}+2gn\right)}}$

For large ${\boldsymbol {q}}$, the dispersion relation is quadratic in ${\boldsymbol {q}}$ as one would expect for usual non interacting single particle excitations. For small ${\boldsymbol {q}}$, the dispersion relation is linear

$\epsilon _{{\boldsymbol {q}}}=s\hbar q$

with $s={\sqrt {ng/m}}$ being the speed of sound in the condensate. The fact that $\epsilon _{{\boldsymbol {q}}}/(\hbar q)>s$ shows, according to Landau's criterion, that the condensate is a superfluid, meaning that if an object is moved in the condensate at a velocity inferior to s, it will not be energetically favorable to produce excitations and the object will move without dissipation, which is a characteristic of a superfluid. Experiments have been done to prove this superfluidity of the condensate, using a tightly focused blue-detuned laser. ^[4] The same dispersion relation is found when the condensate is described from a microscopical approach using the formalism of second quantization.

Superfluid in rotating helical potential

The optical potential well ${\displaystyle V_{twist}({\vec {\mathbf {r} }},t)=V_{twist}(z,r,\theta ,t)}$ might be formed by two counter propagating optical vortices with wavelengths ${\displaystyle \lambda _{\pm }=2\pi c/\omega _{\pm }}$, effective width $D$ and topological charge $\ell$ :

${\displaystyle {E_{\pm }}({\vec {\mathbf {r} }},t)\sim \exp \left(-{\frac {r^{2}}{2D^{2}}}\right)r^{|\ell |}\exp(-i\omega _{\pm }t\pm ik_{\pm }z+i\ell \theta ),}$

where ${\displaystyle \delta \omega =(\omega _{+}-\omega _{-})}$.

In cylindrical coordinate system ${\displaystyle (z,r,\theta )}$ the potential well have a remarkable double helix geometry: ^[5]

${\displaystyle V_{twist}({\vec {\mathbf {r} }},t)\sim V_{0}\exp(-{\frac {r^{2}}{D^{2}}})r^{2|\ell |}\left(1+\cos[\delta \omega t+(k_{+}+k_{-})z+2\ell \theta ]\right),}$

In a reference frame rotating with angular velocity ${\displaystyle \Omega =\delta \omega /2\ell }$, time-dependent Gross–Pitaevskii equation with helical potential is as follows: ^[6]

${\displaystyle i\hbar {\frac {\partial \Psi ({\vec {\mathbf {r} }},t)}{\partial t}}=\left(-{\frac {\hbar ^{2}}{2m}}\nabla ^{2}+V_{twist}({\vec {\mathbf {r} }})+g\vert \Psi ({\vec {\mathbf {r} }},t)\vert ^{2}-\Omega {\hat {L}}\right)\Psi ({\vec {\mathbf {r} }},t),}$

where ${\displaystyle {\hat {L}}=-i\hbar {\frac {\partial }{\partial \theta }}}$ is the angular momentum operator.

The solution for condensate wavefunction ${\displaystyle \Psi ({\vec {\mathbf {r} }},t)}$ is a superposition of two phase-conjugated matter-wave vortices:

${\displaystyle \Psi ({\vec {\mathbf {r} }},t)\sim \exp \left(-{\frac {r^{2}}{2D^{2}}}\right)r^{|\ell |}\times }$

${\displaystyle \left(\exp(-i\omega _{+}t+ik_{+}z+i\ell \theta )+\exp(-i\omega _{-}t-ik_{-}z-i\ell \theta )\right).}$

The macroscopically observable momentum of condensate is :

${\displaystyle \langle \Psi \vert {\hat {P}}\vert \Psi \rangle =N_{at}\hbar (k_{+}-k_{-}),}$

where ${\displaystyle N_{at}}$ is number of atoms in condensate. This means that atomic ensemble moves coherently along ${\displaystyle z-}$ axis with group velocity whose direction is defined by signs of topological charge $\ell$ and angular velocity $\Omega$: ^[7]

${\displaystyle V_{z}={\frac {2\Omega \ell }{(k_{+}+k_{-})}}}$

The angular momentum of helically trapped condensate is exactly zero:^[6]

${\displaystyle \langle \Psi \vert {\hat {L}}\vert \Psi \rangle =N_{at}[\ell \hbar -\ell \hbar ]=0.}$

References

1. E. P. Gross (1961). "Structure of a quantized vortex in boson systems". Il Nuovo Cimento. 20 (3): 454–457. doi:10.1007/BF02731494.
2. L. P. Pitaevskii (1961). "Vortex lines in an imperfect Bose gas". Sov. Phys. JETP. 13 (2): 451–454.
3. N. M. Hugenholtz; D. Pines (1959). "Ground-state energy and excitation spectrum of a system of interacting bosons". Physical Review. 116 (3): 489–506. Bibcode:1959PhRv..116..489H. doi:10.1103/PhysRev.116.489.
4. C. Raman; M. Köhl; R. Onofrio; D. S. Durfee; C. E. Kuklewicz; Z. Hadzibabic; W. Ketterle (1999). "Evidence for a Critical Velocity in a Bose–Einstein Condensed Gas". Phys. Rev. Lett. 83 (13): 2502. doi:10.1103/PhysRevLett.83.2502.
5. A.Yu. Okulov (2008). "Angular momentum of photons and phase conjugation". J. Phys. B: At. Mol. Opt. Phys. 41: 101001. doi:10.1088/0953-4075/41/10/101001.
6. A. Yu. Okulov (2012). "Cold matter trapping via slowly rotating helical potential". Phys. Lett. A. 376 (4): 650–655. doi:10.1016/j.physleta.2011.11.033.
7. A. Yu. Okulov (2013). "Superfluid rotation sensor with helical laser trap". J. Low Temp. Phys. 171 (3): 397–407. doi:10.1007/s10909-012-0837-7.

Further reading

• Pethick, C. J. & Smith, H. (2002). Bose–Einstein Condensation in Dilute Gases. Cambridge: Cambridge University Press. ISBN 0-521-66580-9..
• Pitaevskii, L. P. & Stringari, S. (2003). Bose–Einstein Condensation. Oxford: Clarendon Press. ISBN 0-19-850719-4..

External links

• Trotter-Suzuki-MPI Trotter-Suzuki-MPI is a library for large-scale simulations based on the Trotter-Suzuki decomposition that can also address the Gross–Pitaevskii equation