The Vlasov equation is a differential equation describing time evolution of the distribution function of plasma consisting of charged particles with long-range (for example, Coulomb) interaction. The equation was first suggested for description of plasma by Anatoly Vlasov in 1938[1] (see also [2]) and later discussed by him in detail in a monograph.[3]

Difficulties of the standard kinetic approach

First, Vlasov argues that the standard kinetic approach based on the Boltzmann equation has difficulties when applied to a description of the plasma with long-range Coulomb interaction. He mentions the following problems arising when applying the kinetic theory based on pair collisions to plasma dynamics:

Theory of pair collisions disagrees with the discovery by Rayleigh, Irving Langmuir and Lewi Tonks of natural vibrations in electron plasma.

Theory of pair collisions is formally not applicable to Coulomb interaction due to the divergence of the kinetic terms.

Theory of pair collisions cannot explain experiments by Harrison Merrill and Harold Webb on anomalous electron scattering in gaseous plasma.[4]

Vlasov suggests that these difficulties originate from the long-range character of Coulomb interaction. He starts with the collisionless Boltzmann equation (sometimes anachronistically called the Vlasov equation in this context), in generalized coordinates:

\( \frac{\operatorname df(\mathbf q,\mathbf p,t)}{\operatorname d t} = 0, \)

explicitly a PDE:

\( \frac{\partial f}{\partial t} + \frac {\operatorname d\mathbf {q}}{\operatorname dt} \cdot \frac{\partial f}{\partial \mathbf {q}} + \frac {\operatorname d\mathbf {p}}{\operatorname dt} \cdot \frac{\partial f}{\partial \mathbf {p}} = 0,\)

and adapted it to the case of a plasma, leading to the systems of equations shown below.[5]

The Vlasov–Maxwell system of equations (gaussian units)

Instead of collision-based kinetic description for interaction of charged particles in plasma, Vlasov utilizes a self-consistent collective field created by the charged plasma particles. Such a description uses distribution functions \( f_e(\mathbf {r},\mathbf {p},t) \) and \( f_i(\mathbf {r},\mathbf {p},t)\) for electrons and (positive) plasma ions. The distribution function \( f_{\alpha}(\mathbf {r},\mathbf {p},t) \) for species α describes the number of particles of the species α having approximately the momentum \( \mathbf {p}\) near the position \( \mathbf {r}\) at time t. Instead of the Boltzmann equation, the following system of equations was proposed for description of charged components of plasma (electrons and positive ions):

\( \begin{align} \frac{\partial f_e}{\partial t} + \mathbf {v}_e\cdot\nabla f_e &- e\left(\mathbf {E}+\frac{\mathbf {v_e}}{c}\times\mathbf {B}\right)\cdot\frac{\partial f_e}{\partial\mathbf {p}} = 0 \\ \frac{\partial f_i}{\partial t} + \mathbf {v}_i\cdot\nabla f_i &+ Z_i e\left(\mathbf {E}+\frac{\mathbf {v_i}}{c}\times\mathbf {B}\right)\cdot\frac{\partial f_i}{\partial\mathbf {p}} = 0 \\ \nabla\times\mathbf {B} &=\frac{4\pi\mathbf {j}}{c}+\frac{1}{c}\frac{\partial\mathbf {E}}{\partial t} \\ \nabla\times\mathbf {E} &=-\frac{1}{c}\frac{\partial\mathbf {B}}{\partial t} \\ \nabla\cdot\mathbf {E} &=4\pi\rho \\ \nabla\cdot\mathbf {B} &=0 \\ \end{align}\)

\( \rho=e\int(Z_i f_i-f_e)d^3p,\quad \mathbf {j}=e\int(Z_i f_i \mathbf{v}_i -f_e \mathbf{v}_e)d^3p,\quad \mathbf {v}_\alpha = \frac{\frac{\mathbf {p}}{m_\alpha}}{\left (1+\frac{p^2}{(m_\alpha c)^2}\right )^{1/2}}\)

Here e is the electron charge, c is the speed of light, mi is the mass of the ion, \( \mathbf {E}(\mathbf {r},t)\) and \( \mathbf {B}(\mathbf {r},t)\) represent collective self-consistent electromagnetic field created in the point \( \mathbf {r} at time moment t by all plasma particles. The essential difference of this system of equations from equations for particles in an external electromagnetic field is that the self-consistent electromagnetic field depends in a complex way on the distribution functions of electrons and ions \( f_e(\mathbf {r},\mathbf {p},t)\) and \( f_i(\mathbf {r},\mathbf {p},t)\) .

The Vlasov–Poisson equation

The Vlasov–Poisson equations are an approximation of the Vlasov–Maxwell equations in the nonrelativistic zero-magnetic field limit:

\( \frac{\partial f_{\alpha}}{\partial t} + \mathbf {v}_{\alpha} \cdot \frac{\partial f_{\alpha}}{\partial \mathbf {x}}+ \frac{q_{\alpha}\mathbf {E}}{m_{\alpha}} \cdot \frac{\partial f_{\alpha}}{\partial \mathbf {v}} = 0,\)

and Poisson's equation for self-consistent electric field:

\( \nabla^2 \phi + \rho = 0.\)

Here qα is the particle's electric charge, mα is the particle's mass, \(\mathbf {E}(\mathbf {x},t)\) is the self-consistent electric field, \( \phi(\mathbf {x}, t)\) the self-consistent electric potential and ρ is the electric charge density.

Vlasov–Poisson equations are used to describe various phenomena in plasma, in particular Landau damping and the distributions in a double layer plasma, where they are necessarily strongly non-Maxwellian, and therefore inaccessible to fluid models.

Moment equations

In fluid descriptions of plasmas (see plasma modeling and magnetohydrodynamics (MHD)) one does not consider the velocity distribution. This is achieved by replacing \( f(\mathbf r,\mathbf v,t) \) with plasma moments such as number density n, flow velocity u and pressure p.[6] They are named plasma moments because the n-th moment of f can be found by integrating \( v^n f\) over velocity. These variables are only functions of position and time, which means that some information is lost. In multifluid theory, the different particle species are treated as different fluids with different pressures, densities and flow velocities. The equations governing the plasma moments are called the moment or fluid equations.

Below the two most used moment equations are presented (in SI units). Deriving the moment equations from the Vlasov equation requires no assumptions about the distribution function.

Continuity equation

The continuity equation describes how the density changes with time. It can be found by integration of the Vlasov equation over the entire velocity space.

\( \int\frac{\mathrm d}{\mathrm dt} fd^3v=\int\left(\frac{\partial}{\partial t}f+(\mathbf {v}\cdot\nabla_r)f +\nabla_v\cdot(\mathbf {a}f)\right)d^3v=0 \)

After some calculations, one ends up with

\( \frac{\partial}{\partial t}n+\nabla\cdot (n\mathbf{u})=0.\)

The number density n, and the momentum density nu, are zeroth and first order moments:

\( n = \int f d^3v\)

\( n \mathbf u = \int \mathbf v f d^3v\)

Momentum equation

The rate of change of momentum of a particle is given by the Lorentz equation:

\( m\frac{\mathrm d\mathbf {v}}{\mathrm d t}=q(\mathbf {E} + \mathbf {v}\times\mathbf {B})\)

By using this equation and the Vlasov Equation, the momentum equation for each fluid becomes

\( mn\frac{\mathrm d}{\mathrm d t}\mathbf{u}=-\nabla\cdot\mathbf{p}+qn\mathbf {E}+qn\mathbf{u}\times \mathbf {B},\)

where p is the pressure tensor. The material derivative is

\( \frac{\mathrm D}{\mathrm D t} = \frac{\partial}{\partial t}+\mathbf u\cdot\nabla.\)

The pressure tensor is defined as the particle mass times the covariance matrix of the velocity:

\( p_{ij} = m\int(v_i- u_i)(v_j-u_j)fd^3v.\)

The frozen-in approximation

As for ideal MHD, the plasma can be considered as tied to the magnetic field lines when certain conditions are fulfilled. One often says that the magnetic field lines are frozen into the plasma. The frozen-in conditions can be derived from Vlasov equation.

We introduce the scales T, L and V for time, distance and speed respectively. They represent magnitudes of the different parameters which give large changes in f. By large we mean that

\( \frac{\partial f}{\partial t}T\sim f \quad \left|\frac{\partial f}{\partial\mathbf r}\right|L\sim f \quad\left|\frac{\partial f}{\partial\mathbf v}\right|V\sim f.\)

We then write

\( t^\prime=\frac{t}{T} \quad \mathbf r^\prime=\frac{\mathbf r}{L} \quad \mathbf v^\prime=\frac{\mathbf v}{V}.\)

Vlasov equation can now be written

\( \frac{1}{T}\frac{\partial f}{\partial t^\prime}+\frac{V}{L}\mathbf v^\prime\cdot\frac{\partial f}{\partial \mathbf r^\prime}+\frac{q}{m V}(\mathbf E+V\mathbf v^\prime\times\mathbf B)\cdot\frac{\partial f}{\partial\mathbf v^\prime}=0.\)

So far no approximations have been done. To be able to proceed we set \( V= R\omega_g\) , where \(\omega_g=qB/m\) is the gyro frequency and R is the gyroradius. By dividing by ωg, we get

\( \frac{1}{\omega_gT}\frac{\partial f}{\partial t^\prime}+\frac{R}{L}\mathbf v^\prime\cdot\frac{\partial f}{\partial \mathbf r^\prime}+\left(\frac{\mathbf E}{V B}+\mathbf v^\prime\times\frac{\mathbf B}{B}\right)\cdot\frac{\partial f}{\partial\mathbf v^\prime}=0\)

If \( 1/\omega_g \ll T\) and \( R\ll L, \) the two first terms will be much less than f since \( \partial f/\partial t^\prime\sim f, v^\prime\lesssim 1 \) and \( \partial f/\partial \mathbf r^\prime\sim f\) due to the definitions of T, L and V above. Since the last term is of the order of f, we can neglect the two first terms and write

\( \left(\frac{\mathbf E}{V B}+\mathbf v^\prime\times\frac{\mathbf B}{B}\right)\cdot\frac{\partial f}{\partial\mathbf v^\prime}\approx 0 \Rightarrow (\mathbf E+\mathbf v\times\mathbf B)\cdot\frac{\partial f}{\partial\mathbf v}\approx 0\)

This equation can be decomposed into a field aligned and a perpendicular part:

\( \mathbf E_{\|}\frac{\partial f}{\partial\mathbf v_{\|}}+ (\mathbf E_\perp+\mathbf v\times\mathbf B)\cdot\frac{\partial f}{\partial\mathbf v_\perp}\approx0\)

The next step is to write \( \mathbf \(v=\mathbf v_0+\Delta\mathbf v\) , where

\( \mathbf v_0\times\mathbf B=-\mathbf E_\perp \)

It will soon be clear why this is done. With this substitution, we get

\( \mathbf E_{\|}\frac{\partial f}{\partial\mathbf v_{\|}}+ (\Delta\mathbf v_\perp\times\mathbf B)\cdot\frac{\partial f}{\partial\mathbf v_\perp}\approx0 \)

If the parallel electric field is small,

\( (\Delta\mathbf v_\perp\times\mathbf B)\cdot\frac{\partial f}{\partial\mathbf v_\perp}\approx0 \)

This equation means that the distribution is gyrotropic.[7] The mean velocity of a gyrotropic distribution is zero. Hence, \mathbf v_0 is identical with the mean velocity, u, and we have

\( \mathbf E+\mathbf u\times\mathbf B\approx 0 \)

To summarize, the gyro period and the gyro radius must be much smaller than the typical times and lengths which give large changes in the distribution function. The gyro radius is often estimated by replacing V with the thermal velocity or the Alfvén velocity. In the latter case R is often called the inertial length. The frozen-in conditions must be evaluated for each particle species separately. Because electrons have much smaller gyro period and gyro radius than ions, the frozen-in conditions will more often be satisfied.

Derivation of the Vlasov equation - Peter Pickl

See also

A. A. Vlasov, Many-Particle Theory and Its Application to Plasma, Gordon and Breach, 1961.

List of plasma (physics) articles

References

A. A. Vlasov (1938). "On Vibration Properties of Electron Gas". J. Exp. Theor. Phys. (in Russian) 8 (3): 291.

A. A. Vlasov (1968). "The Vibrational Properties of an Electron Gas". Soviet Physics Uspekhi 10 (6): 721. Bibcode:1968SvPhU..10..721V. doi:10.1070/PU1968v010n06ABEH003709.

A. A. Vlasov (1945). Theory of Vibrational Properties of an Electron Gas and Its Applications.

H. J. Merrill & H. W. Webb (1939). "Electron Scattering and Plasma Oscillations". Physical Review 55 (12): 1191. Bibcode:1939PhRv...55.1191M. doi:10.1103/PhysRev.55.1191.

"Vlasov equation?", M. Hénon, Astronomy and Astrophysics 114, #1 (October 1982), pp. 211-212, Bibcode: 1982A&A...114..211H

W. Baumjohann and R. A. Treumann, Basic Space Plasma Physics, Imperial College Press, 1997

P. C. Clemmow and J. Dougherty, Electrodynamics of Particles and Plasmas, Addison-Wesley series in advanced physics, Addison-Wesley Publishing Company, 1969

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