Screened Poisson equation

In physics, the screened Poisson equation is a partial differential equation, which arises in (for example) Klein–Gordon equation and electric field screening in plasmas.

Statement of the equation

The equation is

$\left[ \Delta - \lambda^2 \right] u(\mathbf{r}) = - f(\mathbf{r}),$

where $\Delta$ is the Laplace operator, λ is a constant, f is an arbitrary function of position (known as the "source function") and u is the function to be determined.

In the homogeneous case (f=0), the screened Poisson equation is the same as the time-independent Klein–Gordon equation. In the inhomogeneous case, the screened Poisson equation is very similar to the inhomogeneous Helmholtz equation, the only difference being the sign within the brackets.

Solutions

Three dimensions

Without loss of generality, we will take λ to be non-negative. When λ is zero, the equation reduces to Poisson's equation. Therefore, when λ is very small, the solution approaches that of the unscreened Poisson equation, which, in dimension $n=3$, is a superposition of 1/r functions weighted by the source function f:

$u(\mathbf{r})_{(\text{Poisson})} = \iiint \mathrm{d}^3r' \frac{f(\mathbf{r}')}{4\pi |\mathbf{r} - \mathbf{r}'|}.$

On the other hand, when λ is extremely large, u approaches the value f/λ², which goes to zero as λ goes to infinity. As we shall see, the solution for intermediate values of λ behaves as a superposition of screened (or damped) 1/r functions, with λ behaving as the strength of the screening.

The screened Poisson equation can be solved for general f using the method of Green's functions. The Green's function G is defined by

$\left[ \Delta - \lambda^2 \right] G(\mathbf{r}) = - \delta^3(\mathbf{r}).$

Assuming u and its derivatives vanish at large r, we may perform a continuous Fourier transform in spatial coordinates:

$G(\mathbf{k}) = \iiint \mathrm{d}^3r \; G(\mathbf{r}) e^{-i \mathbf{k} \cdot \mathbf{r}}$

where the integral is taken over all space. It is then straightforward to show that

$\left[ k^2 + \lambda^2 \right] G(\mathbf{k}) = 1.$

The Green's function in r is therefore given by the inverse Fourier transform,

$G(\mathbf{r}) = \frac{1}{(2\pi)^3} \; \iiint \mathrm{d}^3\!k \; \frac{e^{i \mathbf{k} \cdot \mathbf{r}}}{k^2 + \lambda^2}.$

This integral may be evaluated using spherical coordinates in k-space. The integration over the angular coordinates is straightforward, and the integral reduces to one over the radial wavenumber $k_r$:

$G(\mathbf{r}) = \frac{1}{2\pi^2 r} \; \int_0^{+\infty} \mathrm{d}k_r \; \frac{k_r \, \sin k_r r }{k_r^2 + \lambda^2}.$

This may be evaluated using contour integration. The result is:

$G(\mathbf{r}) = \frac{e^{- \lambda r}}{4\pi r}.$

The solution to the full problem is then given by

$u(\mathbf{r}) = \int \mathrm{d}^3r' G(\mathbf{r} - \mathbf{r}') f(\mathbf{r}') = \int \mathrm{d}^3r' \frac{e^{- \lambda |\mathbf{r} - \mathbf{r}'|}}{4\pi |\mathbf{r} - \mathbf{r}'|} f(\mathbf{r}').$

As stated above, this is a superposition of screened 1/r functions, weighted by the source function f and with λ acting as the strength of the screening. The screened 1/r function is often encountered in physics as a screened Coulomb potential, also called a "Yukawa potential".

Two dimensions

In two dimensions: In the case of a magnetized plasma, the screened Poisson equation is quasi-2D:

$\left( \Delta_\perp -\frac{1}{\rho^2} \right)u(\mathbf{r}_\perp) = -f(\mathbf{r}_\perp)$

with $\Delta_\perp=\nabla\cdot\nabla_\perp$ and $\nabla_\perp=\nabla-\frac{\mathbf{B}}{B}\cdot \nabla$, with $\mathbf{B}$ the magnetic field and $\rho$ is the (ion) Larmor radius. The two-dimensional Fourier Transform of the associated Green's function is:

$G(\mathbf{k_\perp}) = \iint d^2 r~G(\mathbf{r}_\perp)e^{-i\mathbf{k}_\perp\cdot\mathbf{r}_\perp}.$

The 2D screened Poisson equation yields:

$\left( k_\perp^2 +\frac{1}{\rho^2} \right)G(\mathbf{k}_\perp) = 1$.

The Green's function is therefore given by the inverse Fourier transform:

$G(\mathbf{r}_\perp) = \frac{1}{4\pi^2} \; \iint \mathrm{d}^2\!k \; \frac{e^{i \mathbf{k}_\perp \cdot \mathbf{r}_\perp}}{k_\perp^2 + 1 / \rho^2}.$

This integral can be calculated using polar coordinates in k-space:

$\mathbf{k}_\perp = (k_r\cos(\theta),k_r\sin(\theta))$

The integration over the angular coordinate gives a Bessel function, and the integral reduces to one over the radial wavenumber $k_r$:

$G(\mathbf{r}_\perp) = \frac{1}{2\pi} \; \int_{0}^{+\infty} \mathrm{d}k_r \; \frac{k_r \, J_0(k_r r_\perp)}{k_r^2 + 1 / \rho^2} = \frac{1}{2\pi} K_0(r_\perp \, / \, \rho).$

See also

• Yukawa interaction