# Drude model

The Drude model of electrical conduction was proposed in 1900[1][2] by Paul Drude to explain the transport properties of electrons in materials (especially metals). Basically, Ohm's law was well established and stated that the current J and voltage V driving the current are related to the resistance R of the material. The inverse of the resistance is known as the conductance. When we consider a metal of unit length and unit cross sectional area, the conductance is known as the conductivity, which is the inverse of resistivity. The Drude model attempts to explain the resistivity of a conductor in terms of the scattering of electrons (the carriers of electricity) by the relatively immobile ions in the metal that act like obstructions to the flow of electrons.

Drude model electrons (shown here in blue) constantly bounce between heavier, stationary crystal ions (shown in red).

The model, which is an application of kinetic theory, assumes that the microscopic behaviour of electrons in a solid may be treated classically and behaves much like a pinball machine, with a sea of constantly jittering electrons bouncing and re-bouncing off heavier, relatively immobile positive ions.

The two most significant results of the Drude model are an electronic equation of motion,

${\displaystyle {\frac {d}{dt}}\langle \mathbf {p} (t)\rangle =q\left(\mathbf {E} +{\frac {\langle \mathbf {p} (t)\rangle \times \mathbf {B} }{m}}\right)-{\frac {\langle \mathbf {p} (t)\rangle }{\tau }},}$

and a linear relationship between current density J and electric field E,

${\displaystyle \mathbf {J} =\left({\frac {nq^{2}\tau }{m}}\right)\mathbf {E} .}$

Here t is the time, ⟨p⟩ is the average momentum per electron and q, n, m, and τ are respectively the electron charge, number density, mass, and mean free time between ionic collisions. The latter expression is particularly important because it explains in semi-quantitative terms why Ohm's law, one of the most ubiquitous relationships in all of electromagnetism, should hold.[note 1][3][4]

The model was extended in 1905 by Hendrik Antoon Lorentz (and hence is also known as the Drude–Lorentz model)[citation needed] to give the relation between the thermal conductivity and the electric conductivity of metals (see Lorenz number), and is a classical model. Later it was supplemented with the results of quantum theory in 1933 by Arnold Sommerfeld and Hans Bethe, leading to the Drude–Sommerfeld model.

## History

German physicist Paul Drude proposed his model in 1900 when it was not clear whether atoms existed, and it was not clear what atoms were on a microscopic scale.[5] The first direct proof of atoms through the computation of the Avogadro number from a microscopic model is due to Albert Einstein, the first modern model of atom structure dates to 1904 and the Rutherford model to 1909. Drude starts from the discovery of electrons in 1897 by J.J. Thomson and assumes as a simplistic model of solids that the bulk of the solid is composed of positively charged scattering centers, and a sea of electrons submerge those scattering centers to make the total solid neutral from a charge perspective.[note 2]

In modern terms this is reflected in the valence electron model where the sea of electrons is composed of the valence electrons only,[6] and not the full set of electrons available in the solid, and the scattering centers are the inner shells of tightly bound electrons to the nucleus. The scattering centers had a positive charge equivalent to the valence number of the atoms.[note 3] This similarity added to some computation errors in the Drude paper, ended up providing a reasonable qualitative theory of solids capable of making good predictions in certain cases and giving completely wrong results in others. Whenever people tried to give more substance and detail to the nature of the scattering centers, and the mechanics of scattering, and the meaning of the length of scattering, all these attempts ended in failures.[note 4]

The scattering lengths computed in the Drude model, are of the order of 10 to 100 inter-atomic distances, and also these could not be given proper microscopic explanations. In modern terms, there are experiments in which electrons can travel for meters in a solid in the same manner as they would travel in free space, and this shows how a purely classical model cannot work.[7]

Drude scattering is not electron-electron scattering which is only a secondary phenomenon in the modern theory, neither nuclear scattering given electrons can be at most be absorbed by nuclei. The model remains a bit mute on the microscopic mechanisms, in modern terms this is what is now called the "primary scattering mechanism" where the underlying phenomenon can be different case per case.[note 5]

The model gives better predictions for metals, especially in regards to conductivity,[note 6] and sometimes is called Drude theory of metals. This is because metals have essentially a better approximation to the free electron model, i.e. metals do not have complex band structures, electrons behave essentially as free particles and where, in the case of metals, the effective number of de-localized electrons is essentially the same as the valence number.[note 7]

The same Drude theory, despite inconsistencies which baffled most physicists of the period, was the major one accepted to explain solids until the introduction in 1927 of the Drude-Sommerfeld model.

A few more hints of the correct ingredients of a modern theory of solids was given by the following:

• The Einstein solid model and the Debye model, suggesting that the quantum behaviour of exchanging energy in integral units or quanta was an essential component in the full theory especially with regard to specific heats, where the Drude theory failed.
• In some cases, namely in the Hall effect, the theory was making correct predictions if instead of using a negative charge for the electrons a positive one was used. This is now interpreted as holes (i.e. quasi-particles that behave as positive charge carriers) but at the time of Drude it was rather obscure why this was the case.[note 8]

Drude used Maxwell–Boltzmann statistics for the gas of electrons and for deriving the model, which was the only one available at that time. By replacing the statistics with the correct Fermi Dirac statistics, Sommerfeld significantly improved the predictions of the model, although still having a semi-classical theory that could not predict all results of the modern quantum theory of solids.[note 9]

Nowadays Drude and Sommerfeld models are still significant to understanding the qualitative behaviour of solids and to get a first qualitative understanding of a specific experimental setup.[note 10] This is a generic method in solid state physics, where it is typical to incrementally increase the complexity of the models to give more and more accurate predictions. It is less common to use a full-blown quantum field theory from first principles, given the complexities due to the huge numbers of particles and interactions and the little added value of the extra mathematics involved (considering the incremental gain in numerical precision of the predictions).[8]

## Assumptions

Drude used the kinetic theory of gases applied to the gas of electrons moving on a fixed background of "ions"; this is in contrast with the usual way of applying the theory of gases as a neutral diluted gas with no background. The number density of the electron gas was assumed to be

${\displaystyle n={\frac {N_{\text{A}}Z\rho _{\text{m}}}{A}},}$

where Z is the effective number of de-localized electrons per ion, for which Drude used the valence number, A is the atomic mass number, ${\displaystyle \rho _{\text{m}}}$  is the amount of substance concentration of the "ions", and NA is the Avogadro constant. Considering the average volume available per electron as a sphere:

${\displaystyle {\frac {V}{N}}={\frac {1}{n}}={\frac {4}{3}}\pi r_{\rm {s}}^{3}.}$

The quantity ${\displaystyle r_{\text{s}}}$  is a parameter that describes the electron density and is often of the order of 2 or 3 times the Bohr radius, for alkali metals it ranges from 3 to 6 and some metal compounds it can go up to 10. The densities are of the order of 100 times of a typical classical gas.[note 11]

The core assumptions made in the Drude model are the following:

• Drude applied the kinetic theory of a dilute gas, despite the high densities, therefore ignoring electron–electron and electron–ion interactions aside from collisions.[note 12]
• The Drude model considers the metal to be formed of a collection of positively charged ions from which a number of "free electrons" were detached. These may be thought to be the valence electrons of the atoms that have become delocalized due to the electric field of the other atoms.[note 11]
• The Drude model neglects long-range interaction between the electron and the ions or between the electrons; this is called the independent electron approximation.[note 11]
• The electrons move in straight lines between one collision and another; this is called free electron approximation.[note 11]
• The only interaction of a free electron with its environment was treated as being collisions with the impenetrable ions core.[note 11]
• The average time between subsequent collisions of such an electron is τ, with a memoryless Poisson distribution. The nature of the collision partner of the electron does not matter for the calculations and conclusions of the Drude model.[note 11]
• After a collision event, the distribution of the velocity and direction of an electron is determined by only the local temperature and is independent of the velocity of the electron before the collision event.[note 11] The electron is considered to be immediately at equilibrium with the local temperature after a collision.

Removing or improving upon each of these assumptions gives more refined models, that can more accurately describe different solids:

• Improving the hypothesis of the Maxwell–Boltzmann statistics with the Fermi–Dirac statistics leads to the Drude–Sommerfeld model.
• Improving the hypothesis of the Maxwell–Boltzmann statistics with the Bose–Einstein statistics leads to considerations about the specific heat of integer spin atoms[9] and to the Bose–Einstein condensate.
• A valence band electron in a semiconductor is still essentially a free electron in a delimited energy range (i.e. only a "rare" high energy collision that implies a change of band would behave differently); the independent electron approximation is essentially still valid (i.e. no electron–electron scattering), where instead the hypothesis about the localization of the scattering events is dropped (in layman terms the electron is and scatters all over the place).[10]

## Mathematical treatment

### DC field

The simplest analysis of the Drude model assumes that electric field E is both uniform and constant, and that the thermal velocity of electrons is sufficiently high such that they accumulate only an infinitesimal amount of momentum dp between collisions, which occur on average every τ seconds.[note 1]

Then an electron isolated at time t will on average have been travelling for time τ since its last collision, and consequently will have accumulated momentum

${\displaystyle \Delta \langle \mathbf {p} \rangle =q\mathbf {E} \tau .}$

During its last collision, this electron will have been just as likely to have bounced forward as backward, so all prior contributions to the electron's momentum may be ignored, resulting in the expression

${\displaystyle \langle \mathbf {p} \rangle =q\mathbf {E} \tau .}$

Substituting the relations

${\displaystyle \langle \mathbf {p} \rangle =m\langle \mathbf {v} \rangle ,}$
${\displaystyle \mathbf {J} =nq\langle \mathbf {v} \rangle ,}$

results in the formulation of Ohm's law mentioned above:

${\displaystyle \mathbf {J} =\left({\frac {nq^{2}\tau }{m}}\right)\mathbf {E} .}$

### Time-varying analysis

Drude response of current density to an AC electric field.

The dynamics may also be described by introducing an effective drag force. At time t = t0 + dt the electron's momentum will be:

${\displaystyle \mathbf {p} (t_{0}+dt)=(1-{\frac {dt}{\tau }})[\mathbf {p} (t_{0})+\mathbf {f} (t)dt+O(dt^{2})]+{\frac {dt}{\tau }}(\mathbf {g} (t_{0})+\mathbf {f} (t)dt+O(dt^{2}))}$

where ${\displaystyle \mathbf {f} (t)}$  can be interpreted as generic force (e.g. Lorentz Force) on the carrier or more specifically on the electron. ${\displaystyle \mathbf {g} (t_{0})}$  is the momentum of the carrier with random direction after the collision (i.e. with a momentum ${\displaystyle \langle \mathbf {g} (t_{0})\rangle =0}$ ) and with absolute kinetic energy

${\displaystyle {\frac {\langle |\mathbf {g} (t_{0})|\rangle ^{2}}{2m}}={\frac {3}{2}}KT}$ .

On average, a fraction of ${\displaystyle 1-{\frac {dt}{\tau }}}$  of the electrons will not have experienced another collision, the other fraction that had the collision on average will come out in a random direction and will contribute to the total momentum to only a factor ${\displaystyle {\frac {dt}{\tau }}\mathbf {f} (t)dt}$  which is of second order.[note 13]

With a bit of algebra and dropping terms of order ${\displaystyle dt^{2}}$ , this results in the generic differential equation

${\displaystyle {\frac {d}{dt}}\mathbf {p} (t)=\mathbf {f} (t)-{\frac {\mathbf {p} (t)}{\tau }}}$

The second term is actually an extra drag force or damping term due to the Drude effects.

### Constant electric field

At time t = t0 + dt the average electron's momentum will be

${\displaystyle \langle \mathbf {p} (t_{0}+dt)\rangle =\left(1-{\frac {dt}{\tau }}\right)\left(\langle \mathbf {p} (t_{0})\rangle +q\mathbf {E} \,dt\right),}$

and then

${\displaystyle {\frac {d}{dt}}\langle \mathbf {p} (t)\rangle =q\mathbf {E} -{\frac {\langle \mathbf {p} (t)\rangle }{\tau }},}$

where p denotes average momentum and q the charge of the electrons. This, which is an inhomogeneous differential equation, may be solved to obtain the general solution of

${\displaystyle \langle \mathbf {p} (t)\rangle =q\tau \mathbf {E} (1-e^{-t/\tau })+\langle \mathbf {p(0)} \rangle e^{-t/\tau }}$

for p(t). The steady state solution, dp/dt = 0, is then

${\displaystyle \langle \mathbf {p} \rangle =q\tau \mathbf {E} .}$

As above, average momentum may be related to average velocity and this in turn may be related to current density,

${\displaystyle \langle \mathbf {p} \rangle =m\langle \mathbf {v} \rangle ,}$
${\displaystyle \mathbf {J} =nq\langle \mathbf {v} \rangle ,}$

and the material can be shown to satisfy Ohm's law ${\displaystyle \mathbf {J} =\sigma _{0}\mathbf {E} }$  with a DC-conductivity σ0:

${\displaystyle \sigma _{0}={\frac {nq^{2}\tau }{m}}}$

### AC field

Complex conductivity for different frequencies assuming that τ = 10−5 and that σ0 = 1.

The Drude model can also predict the current as a response to a time-dependent electric field with an angular frequency ω. The complex conductivity is

${\displaystyle \sigma (\omega )={\frac {\sigma _{0}}{1-i\omega \tau }}={\frac {\sigma _{0}}{1+\omega ^{2}\tau ^{2}}}+i\omega \tau {\frac {\sigma _{0}}{1+\omega ^{2}\tau ^{2}}}.}$

Here it is assumed that:

${\displaystyle E(t)=\Re \left(E_{0}e^{i\omega t}\right);}$
${\displaystyle J(t)=\Re \left(\sigma (\omega )E_{0}e^{i\omega t}\right).}$

In engineering, i is generally replaced by −i (or −j ) in all equations, which reflects the phase difference with respect to origin, rather than delay at the observation point traveling in time.

Proof using the equation of motion[note 14] —

Given

${\displaystyle \mathbf {p} (t)=\Re \left(\mathbf {p} (\omega )e^{-i\omega t}\right)}$
${\displaystyle \mathbf {E} (t)=\Re \left(\mathbf {E} (\omega )e^{-i\omega t}\right)}$

And the equation of motion above

${\displaystyle {\frac {d}{dt}}\mathbf {p} (t)=-e\mathbf {E} -{\frac {\mathbf {p} (t)}{\tau }}}$

substituting

${\displaystyle -i\omega \mathbf {p} (\omega )=-e\mathbf {E} (\omega )-{\frac {\mathbf {p} (\omega )}{\tau }}}$

Given

${\displaystyle \mathbf {j} =-ne{\frac {\mathbf {p} }{m}}}$
${\displaystyle \mathbf {j} (t)=\Re \left(\mathbf {j} (\omega )e^{-i\omega t}\right)}$
${\displaystyle \mathbf {j} (\omega )=-ne{\frac {\mathbf {p} (\omega )}{m}}={\frac {(ne^{2}/m)\mathbf {E} (\omega )}{1/\tau -i\omega }}}$

defining the complex conductivity from:

${\displaystyle \mathbf {j} (\omega )=\sigma (\omega )\mathbf {E} (\omega )}$

We have:

${\displaystyle \sigma (\omega )={\frac {\sigma _{0}}{1-i\omega \tau }};\sigma _{0}={\frac {ne^{2}\tau }{m}}}$

The imaginary part indicates that the current lags behind the electrical field. This happens because the electrons need roughly a time τ to accelerate in response to a change in the electrical field. Here the Drude model is applied to electrons; it can be applied both to electrons and holes; i.e., positive charge carriers in semiconductors. The curves for σ(ω) are shown in the graph.

If a sinusoidally varying electric field with frequency ${\displaystyle \omega }$  is applied to the solid, the negatively charged electrons behave as a plasma that tends to move a distance x apart from the positively charged background. As a result, the sample is polarized and there will be an excess charge at the opposite surfaces of the sample.

The dielectric constant of the sample is expressed as

${\displaystyle \varepsilon ={\frac {D}{\varepsilon _{0}E}}=1+{\frac {P}{\varepsilon _{0}E}}}$

where ${\displaystyle D}$  is the electric displacement and ${\displaystyle P}$  is the polarization density.

The polarization density is written as

${\displaystyle P(t)=\Re \left(P_{0}e^{i\omega t}\right)}$

and the polarization density with n electron density is

${\displaystyle P=-nex}$

After a little algebra the relation between polarization density and electric field can be expressed as

${\displaystyle P=-{\frac {ne^{2}}{m\omega ^{2}}}E}$

The frequency dependent dielectric function of the solid is

${\displaystyle \varepsilon (\omega )=1-{\frac {ne^{2}}{\varepsilon _{0}m\omega ^{2}}}}$
Proof using Maxwell's equations[note 15] —

Given the approximations for the ${\displaystyle \sigma (\omega )}$  included above

• we assumed no electromagnetic field: this is always smaller by a factor v/c given the additional Lorentz term ${\displaystyle -{\frac {e\mathbf {p} }{mc}}\times \mathbf {B} }$  in the equation of motion
• we assumed spatially uniform field: this is true if the field does not oscillate considerably across a few mean free paths of electrons. This is typically not the case: the mean free path is of the order of Angstroms corresponding to wavelengths typical of X rays.

Given the Maxwell equations without sources (which are treated separately in the scope of plasma oscillations)

${\displaystyle \nabla \cdot \mathbf {E} =0;\nabla \cdot \mathbf {B} =0}$
${\displaystyle \nabla \times \mathbf {E} =-{\frac {1}{c}}{\frac {\partial \mathbf {B} }{\partial t}};\nabla \times \mathbf {B} ={\frac {4\pi }{c}}\mathbf {j} +{\frac {1}{c}}{\frac {\partial \mathbf {E} }{\partial t}}}$

then

${\displaystyle \nabla \times \nabla \times \mathbf {E} =-\nabla ^{2}\mathbf {E} ={\frac {i\omega }{c}}\nabla \times \mathbf {B} ={\frac {i\omega }{c}}\left({\frac {4\pi \sigma }{c}}\mathbf {E} -{\frac {i\omega }{c}}\mathbf {E} \right)}$

or

${\displaystyle \nabla ^{2}\mathbf {E} ={\frac {\omega ^{2}}{c^{2}}}\left(1+{\frac {4\pi i\sigma }{\omega }}\right)\mathbf {E} }$

which is an electromagnetic wave equation for a continuous homogeneous medium with dielectric constant ${\displaystyle \epsilon (\omega )}$  in the helmoltz form

${\displaystyle -\nabla ^{2}\mathbf {E} ={\frac {\omega ^{2}}{c^{2}}}\epsilon (\omega )\mathbf {E} }$

where the refractive index is ${\displaystyle n(\omega )={\sqrt {\epsilon (\omega )}}}$  and the phase velocity is ${\displaystyle v_{p}={\frac {c}{n(\omega )}}}$  therefore the complex dielectric constant is

${\displaystyle \epsilon (\omega )=\left(1+{\frac {4\pi i\sigma }{\omega }}\right)}$

which in the case ${\displaystyle \omega \tau >>1}$  can be approximated to:

${\displaystyle \epsilon (\omega )=\left(1-{\frac {\omega _{\rm {p}}^{2}}{\omega ^{2}}}\right);\omega _{\rm {p}}^{2}={\frac {4\pi ne^{2}}{m}}}$

At a resonance frequency ${\displaystyle \omega _{\rm {p}}}$ , called the plasma frequency, the dielectric function changes sign from negative to positive and real part of the dielectric function drops to zero.

${\displaystyle \omega _{\rm {p}}={\sqrt {\frac {ne^{2}}{\varepsilon _{0}m}}}}$

The plasma frequency represents a plasma oscillation resonance or plasmon. The plasma frequency can be employed as a direct measure of the square root of the density of valence electrons in a solid. Observed values are in reasonable agreement with this theoretical prediction for a large number of materials.[11] Below the plasma frequency, the dielectric function is negative and the field cannot penetrate the sample. Light with angular frequency below the plasma frequency will be totally reflected. Above the plasma frequency the light waves can penetrate the sample, a typical example are alkaline metals that becomes transparent in the range of ultraviolet radiation. [note 16]

### Thermal conductivity of metals

One great success of the Drude model is the explanation of the Wiedemann-Franz law. This was due to a fortuitous cancellation of errors in Drude's original calculation. Drude predicted the value of the Lorenz number:

${\displaystyle {\frac {\kappa }{\sigma T}}={\frac {3}{2}}\left({\frac {k_{\rm {B}}}{e}}\right)^{2}=1.11\times 10^{-8}\,{\text{W}}\Omega /{\text{K}}^{2}}$

Experimental values are typically in the range of ${\displaystyle 2-3\times 10^{-8}\,{\text{W}}\Omega /{\text{K}}^{2}}$  for metals at temperatures between 0 and 100 degrees Celsius.[note 17]

Derivation and Drude's errors[note 15] —

Solids can conduct heat through the motion of electrons, atoms, and ions. Conductors have a large density of free electrons whereas insulators do not; ions may be present in either. Given the good electrical and thermal conductivity in metals and the poor electrical and thermal conductivity in insulators, a natural starting point to estimate the thermal conductivity is to calculate the contribution of the conduction electrons.

The thermal current density is the flux per unit time of thermal energy across a unit area perpendicular to the flow. It is proportional to the temperature gradient.

${\displaystyle \mathbf {j} _{q}=-\kappa \nabla T}$

where ${\displaystyle \kappa }$  is the thermal conductivity. In a one-dimensional wire, the energy of electrons depends on the local temperature ${\displaystyle \epsilon [T(x)]}$  If we imagine a temperature gradient in which the temperature decreases in the positive x direction, the average electron velocity is zero (but not the average speed). The electrons arriving at location x from the higher-energy side will arrive with energies ${\displaystyle \varepsilon [T(x-v\tau )]}$ , while those from the lower-energy side will arrive with energies ${\displaystyle \varepsilon [T(x+v\tau )]}$ . Here, ${\displaystyle v}$  is the average speed of electrons and ${\displaystyle \tau }$  is the average time since the last collision.

The net flux of thermal energy at location x is the difference between what passes from left to right and from right to left:

${\displaystyle \mathbf {j} _{q}={\frac {1}{2}}nv{\big (}\varepsilon [T(x-v\tau )]-\varepsilon [T(x+v\tau )]{\big )}}$

The factor of 1/2 accounts for the fact that electrons are equally likely to be moving in either direction. Only half contribute to the flux at x.

When the mean free path ${\displaystyle \ell =v\tau }$  is small, the quantity ${\displaystyle {\big (}\varepsilon [T(x-v\tau )]-\varepsilon [T(x+v\tau )]{\big )}/2v\tau }$  can be approximated by a derivative with respect to x. This gives

${\displaystyle \mathbf {j} _{q}=nv^{2}\tau {\frac {d\varepsilon }{dT}}\cdot (-{\frac {dT}{dx}})}$

Since the electron moves in the ${\displaystyle x}$ , ${\displaystyle y}$ , and ${\displaystyle z}$  directions, the mean square velocity in the ${\displaystyle x}$  direction is ${\displaystyle \langle v_{x}^{2}\rangle ={\tfrac {1}{3}}\langle v^{2}\rangle }$ . We also have ${\displaystyle n{\frac {d\varepsilon }{dT}}={\frac {N}{V}}{\frac {d\varepsilon }{dT}}={\frac {1}{V}}{\frac {dE}{dT}}=c_{v}}$ , where ${\displaystyle c_{v}}$  is the specific heat capacity of the material.

Putting all of this together, the thermal energy current density is

${\displaystyle \mathbf {j} _{q}=-{\frac {1}{3}}v^{2}\tau c_{v}\nabla T}$

This determines the thermal conductivity:

${\displaystyle \kappa ={\frac {1}{3}}v^{2}\tau c_{v}}$

(This derivation ignores the temperature-dependence, and hence the position-dependence, of the speed v. This will not introduce a significant error unless the temperature changes rapidly over a distance comparable to the mean free path.)

Dividing the thermal conductivity ${\displaystyle \kappa }$  by the electrical conductivity ${\displaystyle \sigma ={\frac {ne^{2}\tau }{m}}}$  eliminates the scattering time ${\displaystyle \tau }$  and gives

${\displaystyle {\frac {\kappa }{\sigma }}={\frac {c_{v}mv^{2}}{3ne^{2}}}}$

At this point of the calculation, Drude made two assumptions now known to be errors. First, he used the classical result for the specific heat capacity of the conduction electrons: ${\displaystyle c_{v}={\tfrac {3}{2}}nk_{\rm {B}}}$ . This overestimates the electronic contribution to the specific heat capacity by a factor of roughly 100. Second, Drude used the classical mean square velocity for electrons, ${\displaystyle {\tfrac {1}{2}}mv^{2}={\tfrac {3}{2}}k_{\rm {B}}T}$ . This underestimates the energy of the electrons by a factor of roughly 100. The cancellation of these two errors results in a good approximation to the conductivity of metals. In addition to these two estimates, Drude also made a statistical error and overestimated the mean time between collisions by a factor of 2. This confluence of errors gave a value for the Lorenz number that was remarkably close to experimental values.

The correct value of the Lorenz number as estimated from the Drude model is

${\displaystyle {\frac {\kappa }{\sigma T}}={\frac {3}{2}}\left({\frac {k_{\rm {B}}}{e}}\right)^{2}=1.11\times 10^{-8}\,{\text{W}}\Omega /{\text{K}}^{2}}$ .

[note 18]

### Thermopower

A generic temperature gradient when switched on in a thin bar will trigger a current of electrons towards the lower temperature side, given the experiments are done in an open circuit manner this current will accumulate on that side generating an electric field countering the electric current. This field is called thermoelectric field:

${\displaystyle \mathbf {E} =Q\nabla T}$

and Q is called thermopower. The estimates by Drude are a factor of 100 low given the direct dependency with the specific heat.

${\displaystyle Q=-{\frac {c_{v}}{3ne}}=-{\frac {k_{\rm {B}}}{2e}}=0.43\times 10^{-4}{\text{V}}/{\text{K}}}$

where the typical thermopowers at room temperature are 100 times smaller of the order of micro-volts.[note 19]

Proof together with the Drude errors[note 20] —

From the simple one dimensional model

${\displaystyle v_{Q}={\frac {1}{2}}[v(x-v\tau )-v(x+v\tau )]=-v\tau {\frac {dv}{dx}}=-\tau {\frac {d}{dx}}\left({\frac {v^{2}}{2}}\right)}$

Expanding to 3 degrees of freedom ${\displaystyle \langle v_{x}^{2}\rangle ={\frac {1}{3}}\langle v^{2}\rangle }$

${\displaystyle \mathbf {v_{Q}} =-{\frac {\tau }{6}}{\frac {dv^{2}}{dT}}(\nabla T)}$

The mean velocity due to the Electric field (given the equation of motion above at equilibrium)

${\displaystyle \mathbf {v_{E}} =-{\frac {e\mathbf {E} \tau }{m}}}$

To have a total current null ${\displaystyle \mathbf {v_{E}} +\mathbf {v_{Q}} =0}$  we have

${\displaystyle Q=-{\frac {1}{3e}}{\frac {d}{dT}}\left({\frac {mv^{2}}{2}}\right)=-{\frac {c_{v}}{3ne}}}$

And as usual in the Drude case ${\displaystyle c_{v}={\frac {3}{2}}nk_{\rm {B}}}$

${\displaystyle Q=-{\frac {k_{\rm {B}}}{2e}}=0.43\times 10^{-4}{\text{V}}/{\text{K}}}$

where the typical thermopowers at room temperature are 100 times smaller of the order of micro-Volts.[note 19]

## Drude response in real materials

The characteristic behavior of a Drude metal in the time or frequency domain, i.e. exponential relaxation with time constant τ or the frequency dependence for σ(ω) stated above, is called Drude response. In a conventional, simple, real metal (e.g. sodium, silver, or gold at room temperature) such behavior is not found experimentally, because the characteristic frequency τ−1 is in the infrared frequency range, where other features that are not considered in the Drude model (such as band structure) play an important role.[12] But for certain other materials with metallic properties, frequency-dependent conductivity was found that closely follows the simple Drude prediction for σ(ω). These are materials where the relaxation rate τ−1 is at much lower frequencies.[12] This is the case for certain doped semiconductor single crystals,[13] high-mobility two-dimensional electron gases,[14] and heavy-fermion metals.[15]

## Accuracy of the model

Historically, the Drude formula was first derived in a limited way, namely by assuming that the charge carriers form a classical ideal gas. Arnold Sommerfeld considered quantum theory and extended the theory to the free electron model, where the carriers follow Fermi–Dirac distribution. The conductivity predicted is the same as in the Drude model because it does not depend on the form of the electronic speed distribution.

The Drude model provides a very good explanation of DC and AC conductivity in metals, the Hall effect, and the magnetoresistance[note 13] in metals near room temperature. The model also explains partly the Wiedemann–Franz law of 1853. However, it greatly overestimates the electronic heat capacities of metals. In reality, metals and insulators have roughly the same heat capacity at room temperature.

The model can also be applied to positive (hole) charge carriers.

In his original paper, Drude made an error, estimating the Lorenz number of Wiedemann–Franz law to be twice what it classically should have been, thus making it seem in agreement with the experimental value of the specific heat. This number is about 100 times smaller than the classical prediction but this factor cancels out with the mean electronic speed that is about 100 times bigger than Drude's calculation.[note 21]

## Citations

1. ^ a b Ashcroft & Mermin 1976, pp. 6–7
2. ^ Ashcroft & Mermin 1976, pp. 2–3
3. ^ Ashcroft & Mermin 1976, pp. 3 page note 4 and fig. 1.1
4. ^ Ashcroft & Mermin 1976, pp. 3 page note 7 and fig. 1.2
5. ^ Ashcroft & Mermin 1976, pp. 3 page note 6
6. ^ Ashcroft & Mermin 1976, pp. 8 table 1.2
7. ^ Ashcroft & Mermin 1976, pp. 5 table 1.1
8. ^ Ashcroft & Mermin 1976, pp. 15 table 1.4
9. ^ Ashcroft & Mermin 1976, pp. 4
10. ^ Ashcroft & Mermin 1976, pp. 2
11. Ashcroft & Mermin 1976, pp. 2–6
12. ^ Ashcroft & Mermin 1976, pp. 4
13. ^ a b Ashcroft & Mermin 1976, p. 11
14. ^ Ashcroft & Mermin 1976, pp. 16
15. ^ a b Ashcroft & Mermin 1976, pp. 17
16. ^ Ashcroft & Mermin 1976, pp. 18 table 1.5
17. ^ Ashcroft & Mermin 1976, pp. 18 table 1.6
18. ^ Ashcroft & Mermin 1976, pp. 25 prob 1
19. ^ a b Ashcroft & Mermin 1976, pp. 25
20. ^ Ashcroft & Mermin 1976, pp. 24
21. ^ Ashcroft & Mermin 1976, p. 23

## References

1. ^ Drude, Paul (1900). "Zur Elektronentheorie der Metalle". Annalen der Physik. 306 (3): 566–613. Bibcode:1900AnP...306..566D. doi:10.1002/andp.19003060312.
2. ^ Drude, Paul (1900). "Zur Elektronentheorie der Metalle; II. Teil. Galvanomagnetische und thermomagnetische Effecte". Annalen der Physik. 308 (11): 369–402. Bibcode:1900AnP...308..369D. doi:10.1002/andp.19003081102.
3. ^ Edward M. Purcell (1965). Electricity and Magnetism. McGraw-Hill. pp. 117–122. ISBN 978-0-07-004908-6.
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