View source for Reciprocity (electromagnetism)

{{Short description|Theorem in classical electromagnetism}}
{{about|reciprocity theorems in classical electromagnetism|unrelated reciprocity theorems|Reciprocity theorem (disambiguation)|more general usages of the term|Reciprocity (disambiguation)}}
{{Electromagnetism}}

In [[Maxwell's equations|classical electromagnetism]], '''reciprocity''' refers to a variety of related theorems involving the interchange of time-[[harmonic (mathematics)|harmonic]] electric [[current density|current densities]] (sources) and the resulting [[electromagnetic field]]s in [[Maxwell's equations]] for time-invariant linear media under certain constraints. Reciprocity is closely related to the concept of [[Hermitian operator|symmetric operator]]s from [[linear algebra]], applied to electromagnetism.

Perhaps the most common and general such theorem is '''Lorentz reciprocity''' (and its various special cases such as '''Rayleigh-Carson reciprocity'''),  named after work by [[Hendrik Lorentz]] in 1896 following analogous results regarding [[sound]] by [[Lord Rayleigh]] and [[light]] by [[Helmholtz]] (Potton, 2004). Loosely, it states that the relationship between an oscillating current and the resulting [[electric field]] is unchanged if one interchanges the points where the current is placed and where the field is measured.  For the specific case of an [[electrical network]], it is sometimes phrased as the statement that [[voltage]]s and [[Current (electricity)|current]]s at different points in the network can be interchanged. More technically, it follows that the mutual [[Electrical impedance|impedance]] of a first circuit due to a second is the same as the mutual impedance of the second circuit due to the first.

Reciprocity is useful in [[optics]], which (apart from quantum effects) can be expressed in terms of classical electromagnetism, but also in terms of [[radiometry]].

There is also an analogous theorem in [[electrostatics]], known as '''Green's reciprocity''', relating the interchange of [[electric potential]] and [[electric charge density]].

Forms of the reciprocity theorems are used in many electromagnetic applications, such as analyzing electrical networks and [[antenna (radio)|antenna]] systems.<ref>
{{cite book
 |first=M. |last=Stumpf
 |year=2018
 |title=Electromagnetic Reciprocity in Antenna Theory
 |publisher=Wiley-IEEE Press
 |place=Piscataway, NJ
}}
</ref>
For example, reciprocity implies that antennas work equally well as transmitters or receivers, and specifically that an antenna's [[radiation pattern|radiation and receiving patterns]] are identical. Reciprocity is also a basic lemma that is used to prove other theorems about electromagnetic systems, such as the symmetry of the [[impedance parameters|impedance matrix]] and [[scattering parameters|scattering matrix]], symmetries of [[Green's function]]s for use in [[Method of moments (electromagnetics)|boundary-element]] and transfer-matrix computational methods, as well as [[orthogonality]] properties of [[harmonic mode]]s in [[waveguide]] systems (as an alternative to proving those properties directly from the symmetries of the [[Eigenvalue, eigenvector and eigenspace|eigen-operators]]).

== Lorentz reciprocity ==
Specifically, suppose that one has a current density <math> \mathbf{J}_1 </math> that produces an [[electric field]] <math> \mathbf{E}_1 </math> and a [[magnetic field]] <math> \mathbf{H}_1\, ,</math> where all three are periodic functions of time with [[angular frequency]] {{mvar|ω}}, and in particular they have time-dependence <math> \exp(-i\omega t)\, .</math> Suppose that we similarly have a second current <math> \mathbf{J}_2 </math> at the same frequency {{mvar|ω}} which (by itself) produces fields <math> \mathbf{E}_2 </math> and <math> \mathbf{H}_2\, .</math> The Lorentz reciprocity theorem then states, under certain simple conditions on the materials of the medium described below, that for an arbitrary surface {{mvar|S}} enclosing a volume {{mvar|V}}:

:<math>\int_V \left[ \mathbf{J}_1 \cdot \mathbf{E}_2 - \mathbf{E}_1 \cdot \mathbf{J}_2 \right] \mathrm{d}V = \oint_S \left[ \mathbf{E}_1 \times \mathbf{H}_2 - \mathbf{E}_2 \times \mathbf{H}_1 \right] \cdot \mathbf{\mathrm{d}S}\ .</math>

Equivalently, in differential form (by the [[divergence theorem]]):

:<math> \mathbf{J}_1 \cdot \mathbf{E}_2 - \mathbf{E}_1 \cdot \mathbf{J}_2 = \nabla \cdot \left[ \mathbf{E}_1 \times \mathbf{H}_2 - \mathbf{E}_2 \times \mathbf{H}_1 \right]\ .</math>

This general form is commonly simplified for a number of special cases. In particular, one usually assumes that <math>\ \mathbf{J}_1\ </math> and <math>\mathbf{J}_2</math> are localized (i.e. have [[compact support]]), and that there are no incoming waves from infinitely far away.  In this case, if one integrates throughout space then the surface-integral terms cancel (see below) and one obtains:

:<math> \int \mathbf{J}_1 \cdot \mathbf{E}_2 \, \mathrm{d}V = \int \mathbf{E}_1 \cdot \mathbf{J}_2 \, \mathrm{d}V\ .</math>

This result (along with the following simplifications) is sometimes called the '''Rayleigh-Carson reciprocity theorem''', after Lord Rayleigh's work on sound waves and an extension by [[John R. Carson|Carson]] (1924; 1930) to applications for [[radio frequency]] antennas. Often, one further simplifies this relation by considering point-like [[dipole]] sources, in which case the integrals disappear and one simply has the product of the electric field with the corresponding dipole moments of the currents. Or, for wires of negligible thickness, one obtains the applied current in one wire multiplied by the resulting voltage across another and vice versa; see also below.

Another special case of the Lorentz reciprocity theorem applies when the volume {{mvar|V}} entirely contains ''both'' of the localized sources (or alternatively if {{mvar|V}} intersects ''neither'' of the sources). In this case:

:<math>\ \oint_S (\mathbf{E}_1 \times \mathbf{H}_2) \cdot \mathbf{\mathrm{d}S} = \oint_S (\mathbf{E}_2 \times \mathbf{H}_1) \cdot \mathbf{\mathrm{d}S} \ .</math>

In practical problems, there are another more generalized forms of Lorentz and other reciprocity relations, in which, in addition to [[Current density|electric current density]] <math>\ \mathbf{J}\ </math>, [[magnetic current|magnetic current density]] <math>\ \mathbf{M}\ </math> is also used. These types of reciprocity relations are usually discussed in [[electrical engineering]] literature.<ref>{{cite book | last=Balanis | first=C. A. | author-link=Constantine A. Balanis | title=Advanced Engineering Electromagnetics | publisher=[[Wiley (publisher)|Wiley]] | edition=3 | pages=335-337 | date=2024 | isbn=978-1-394-18001-1 | doi=10.1002/9781394180042 | url=https://www.wiley.com/en-us/Balanis%27+Advanced+Engineering+Electromagnetics%2C+3rd+Edition-p-9781394180011 | access-date=February 29, 2024}}</ref><ref>{{cite book | last=Harrington | first=R. F. | author-link=Roger F. Harrington | title=Time-Harmonic Electromagnetic Fields | publisher=[[Wiley (publisher)|Wiley]]-[[Institute of Electrical and Electronics Engineers|IEEE]] | pages=116-120 | date=2001 | isbn=978-0-471-20806-8 | doi=10.1109/9780470546710 | url=https://www.wiley.com/en-us/Time+Harmonic+Electromagnetic+Fields-p-9780471208068 | access-date=February 29, 2024}}</ref><ref>{{cite book | last=Van Bladel | first=J. | author-link=Jean van Bladel | title=Electromagnetic Fields | publisher=[[Wiley (publisher)|Wiley]]-[[Institute of Electrical and Electronics Engineers|IEEE]] | edition=2 | pages=397-402 | date=2007 | isbn=978-0-471-26388-3 | doi=10.1002/047012458X | url=https://www.wiley.com/en-us/Electromagnetic+Fields%2C+2nd+Edition-p-9780471263883 | access-date=February 29, 2024}}</ref><ref>{{cite book | last1=Felsen | first1=L. B. | author1-link=Leopold B. Felsen | last2=Marcuvitz | first2=N. | author2-link=Nathan Marcuvitz | title=Radiation and Scattering of Waves | publisher=[[Wiley (publisher)|Wiley]]-[[Institute of Electrical and Electronics Engineers|IEEE]] | pages=90-93 | date=2003 | isbn=978-0-780-31088-9 | doi=10.1109/9780470546307 | url=https://www.wiley.com/en-us/Radiation+and+Scattering+of+Waves-p-9780780310889 | access-date=February 29, 2024}}</ref><ref>{{cite book | last=Collin | first=R. E. | author-link=Robert E. Collin | title=Field Theory of Guided Waves | publisher=[[Wiley (publisher)|Wiley]]-[[Institute of Electrical and Electronics Engineers|IEEE]] | edition=2 | pages=49-50 | date=1991 | isbn=978-0-879-42237-0 | doi=10.1109/9780470544648 | url=https://www.wiley.com/en-us/Field+Theory+of+Guided+Waves%2C+2nd+Edition-p-9780879422370 | access-date=February 29, 2024}}</ref>

== Reciprocity for electrical networks ==
{{see also|Reciprocity (electrical networks)}}

Above, Lorentz reciprocity was phrased in terms of an externally applied current source and the resulting field. Often, especially for electrical networks, one instead prefers to think of an externally applied voltage and the resulting currents. The Lorentz reciprocity theorem describes this case as well, assuming [[Ohm's law|ohmic materials]] (i.e. currents that respond linearly to the applied field) with a 3×3 [[Electrical conductivity|conductivity]] matrix {{mvar|σ}} that is required to be [[symmetric matrix|symmetric]], which is implied by the other conditions below.  In order to properly describe this situation, one must carefully distinguish between the externally ''applied'' fields (from the driving voltages) and the ''total'' fields that result (King, 1963).

More specifically, the <math>\ \mathbf{J}\ </math> above only consisted of external "source" terms introduced into Maxwell's equations. We now denote this by <math>\ \mathbf{J}^{(e)}\ </math> to distinguish it from the ''total'' current produced by both the external source and by the resulting electric fields in the materials. If this external current is in a material with a conductivity {{mvar|σ}}, then it corresponds to an externally applied electric field <math>\ \mathbf{E}^{(e)}\ </math> where, by definition of {{mvar|σ}}:

:<math>\ \mathbf{J}^{(e)}=\sigma\mathbf{E}^{(e)}\ .</math>

Moreover, the electric field <math>\mathbf{E}</math> above only consisted of the ''response'' to this current, and did not include the "external" field <math>\ \mathbf{E}^{(e)}\ .</math> Therefore, we now denote the field from before as <math>\ \mathbf{E}^{(r)}\ ,</math> where the ''total'' field is given by <math>\ \mathbf{E} = \mathbf{E}^{(e)} + \mathbf{E}^{(r)}\ .</math> 

Now, the equation on the left-hand side of the Lorentz reciprocity theorem can be rewritten by moving the {{mvar|σ}} from the external current term <math>\mathbf{J}^{(e)}</math> to the response field terms <math>\ \mathbf{E}^{(r)}\ ,</math> and also adding and subtracting a <math>\ \sigma\mathbf{E}_1^{(e)}\mathbf{E}_2^{(e)}\ </math> term, to obtain the external field multiplied by the ''total'' current <math>\ \mathbf{J} = \sigma\mathbf{E}\ :</math>

:<math>\begin{align}
       &\int_V \left[ \mathbf{J}_1^{(e)} \cdot \mathbf{E}_2^{(r)} - \mathbf{E}_1^{(r)} \cdot \mathbf{J}_2^{(e)} \right] \operatorname{d}V \\
  = {} &\int_V \left[ \sigma \mathbf{E}_1^{(e)} \cdot \left(\mathbf{E}_2^{(r)} + \mathbf{E}_2^{(e)}\right) - \left(\mathbf{E}_1^{(r)} + \mathbf{E}_1^{(e)}\right) \cdot \sigma\mathbf{E}_2^{(e)} \right] \operatorname{d}V \\
  = {} &\int_V \left[ \mathbf{E}_1^{(e)} \cdot \mathbf{J}_2 - \mathbf{J}_1 \cdot \mathbf{E}_2^{(e)} \right] \operatorname{d}V\ .
\end{align}</math>

For the limit of thin wires, this gives the product of the externally applied voltage (1) multiplied by the resulting total current (2) and vice versa. In particular, the Rayleigh-Carson reciprocity theorem becomes a simple summation:

:<math>\ \sum_n \mathcal{V}_1^{(n)} I_2^{(n)} = \sum_n \mathcal{V}_2^{(n)} I_1^{(n)} </math>

where <math>\ \mathcal{V}\ </math> and {{mvar|I}} denote the [[complex amplitudes]] of the [[alternating current|AC]] applied voltages and the resulting currents, respectively, in a set of circuit elements (indexed by {{mvar|n}}) for two possible sets of voltages <math>\ \mathcal{V}_1\ </math> and <math>\ \mathcal{V}_2\ .</math> 

Most commonly, this is simplified further to the case where each system has a ''single'' voltage source <math>\ \mathcal{V}_\text{s}\ ,</math> at <math>\ \mathcal{V}_1^{(1)} = \mathcal{V}_\text{s}\ </math> and <math>\ \mathcal{V}_2^{(2)} = \mathcal{V}_\text{s}\ .</math> Then the theorem becomes simply
:<math> I_1^{(2)} = I_2^{(1)} </math>

or in words:
:''The current at position (1) from a voltage at (2) is identical to the current at (2) from the same voltage at (1).''

==Conditions and proof of Lorentz reciprocity==
The Lorentz reciprocity theorem is simply a reflection of the fact that the linear operator <math> \operatorname{\hat{O}} </math> relating <math> \mathbf{J} </math> and <math> \mathbf{E} </math> at a fixed frequency <math> \omega </math> (in linear media):
<math display="block"> \mathbf{J} = \operatorname{\hat{O}} \mathbf{E} </math>
where
<math display="block">  \operatorname{\hat{O}} \mathbf{E} \equiv \frac{1}{i\omega} \left[ \frac{1}{\mu} \left( \nabla \times \nabla \times \right) - \; \omega^2 \varepsilon \right] \mathbf{E} </math>
is usually a [[Hermitian operator|symmetric operator]] under the "[[inner product]]" <math display="inline"> (\mathbf{F}, \mathbf{G}) = \int \mathbf{F} \cdot \mathbf{G} \, \mathrm{d}V</math> for [[vector field]]s <math> \mathbf{F} </math> and <math> \mathbf{G}\ .</math><ref>
{{cite journal
 | last=Chew  | first=Wen Cho
 | date=April 2008
 | title=A new look at reciprocity and energy conservation theorems in electromagnetics
 | journal=IEEE Transactions on Antennas and Propagation
 | volume=56  | issue=4  | pages =970–975
 | doi=10.1109/TAP.2008.919189
| bibcode=2008ITAP...56..970C
 | s2cid=13615400
 }}
</ref>
(Technically, this [[Complex conjugate|unconjugated]] form is not a true inner product because it is not real-valued for complex-valued fields, but that is not a problem here. In this sense, the operator is not truly Hermitian but is rather complex-symmetric.) This is true whenever the [[permittivity]] {{mvar|ε}} and the [[magnetic permeability]] {{mvar|μ}}, at the given {{mvar|ω}}, are [[symmetric matrix|symmetric]] 3×3 matrices (symmetric rank-2 tensors) – this includes the common case where they are [[scalar (physics)|scalar]]s (for isotropic media), of course. They need ''not'' be real – complex values correspond to materials with losses, such as conductors with finite conductivity {{mvar|σ}} (which is included in {{mvar|ε}} via <math> \varepsilon \rightarrow \varepsilon + i\sigma/\omega\ </math>) – and because of this, the reciprocity theorem does ''not'' require [[time reversal invariance]]. The condition of symmetric {{mvar|ε}} and {{mvar|μ}} matrices is almost always satisfied; see below for an exception.

For any Hermitian operator <math> \operatorname{\hat{O}} </math> under an inner product <math>(f,g)\!</math>, we have <math> (f,\operatorname{\hat{O}}g) = (\operatorname{\hat{O}}f,g) </math> by definition, and the Rayleigh-Carson reciprocity theorem is merely the vectorial version of this statement for this particular operator <math> \mathbf{J} = \operatorname{\hat{O}} \mathbf{E}\ :</math> that is, <math> (\mathbf{E}_1, \operatorname{\hat{O}}\mathbf{E}_2) = (\operatorname{\hat{O}} \mathbf{E}_1, \mathbf{E}_2)\ .</math> The Hermitian property of the operator here can be derived by [[integration by parts]]. For a finite integration volume, the surface terms from this integration by parts yield the more-general surface-integral theorem above. In particular, the key fact is that, for vector fields <math> \mathbf{F} </math> and <math> \mathbf{G}\ ,</math> integration by parts (or the [[divergence theorem]]) over a volume {{mvar|V}} enclosed by a surface {{mvar|S}} gives the identity:
<math display="block">\int_V \mathbf{F} \cdot (\nabla\times\mathbf{G}) \, \mathrm{d}V \equiv \int_V (\nabla\times\mathbf{F}) \cdot \mathbf{G} \, \mathrm{d}V - \oint_S (\mathbf{F} \times \mathbf{G}) \cdot \mathrm{d}\mathbf{A}\ .</math>

This identity is then applied twice to <math> (\mathbf{E}_1, \operatorname{\hat{O}} \mathbf{E}_2) </math> to yield <math> (\operatorname{\hat{O}} \mathbf{E}_1, \mathbf{E}_2) </math> plus the surface term, giving the Lorentz reciprocity relation.

;Conditions and proof of Lorenz reciprocity using Maxwell's equations and vector operations<ref>
{{cite book
 |author1=Ramo, Simon
 |author2=Whinnery, John
 |author3=van&nbsp;Duzer, Theodore
 |year=1965
 |title=Fields and Waves in Communication Electronics
 |publisher=John Wiley & Sons
 |isbn=978-047170720-2
 |edition=International
}}
{{isbn|0471707201}}
</ref>

We shall prove a general form of the electromagnetic reciprocity theorem due to Lorenz which states that fields <math>\mathbf {E}_1, \mathbf {H}_1</math> and <math>\mathbf {E}_2, \mathbf {H}_2</math> generated by two different sinusoidal current densities respectively <math>\mathbf {J}_1</math> and <math> \mathbf {J}_2 </math> of the same frequency, satisfy the condition 
<math display="block"> \int_V \left[ \mathbf{J}_1 \cdot \mathbf{E}_2 - \mathbf{E}_1 \cdot \mathbf{J}_2 \right] \mathrm{d}V = \oint_S \left[ \mathbf{E}_1 \times \mathbf{H}_2 - \mathbf{E}_2 \times \mathbf{H}_1 \right] \cdot \mathbf{\mathrm{d}S} .</math>  

Let us take a region in which dielectric constant and permeability may be functions of position but not of time. Maxwell's equations, written in terms of the total fields, currents and charges of the region describe the electromagnetic behavior of the region. The two curl equations are:
<math display="block">\begin{array}{ccc}
\nabla\times\mathbf E & = & - \frac{\partial}{\partial t}\mathbf B\ ,\\
\nabla\times\mathbf H & = & \mathbf J + \frac{\partial}{\partial t}\mathbf D\ .
\end{array}</math>

Under steady constant frequency conditions we get from the two curl equations the Maxwell's equations for the Time-Periodic case:
<math display="block">\begin{array}{ccc}
\nabla\times\mathbf E & = & - j\omega\mathbf B\ ,\\
\nabla\times\mathbf H & = & \mathbf J + j\omega\mathbf D\ .
\end{array}</math>

It must be recognized that the symbols in the equations of this article represent the complex multipliers of <math> e^{j\omega t} </math>, giving the in-phase and out-of-phase parts with respect to the chosen reference. The complex vector multipliers of <math> e^{j\omega t} </math> may be called ''vector phasors'' by analogy to the complex scalar quantities which are commonly referred to as ''phasors''.

An equivalence of vector operations shows that 
<math display="block"> \mathbf H\cdot(\nabla \times \mathbf E) - \mathbf E \cdot (\nabla \times \mathbf H) = \nabla \cdot (\mathbf E \times \mathbf H) </math> for every vectors <math> \mathbf E </math> and <math> \mathbf H\ .</math>

If we apply this equivalence to <math> \mathbf {E}_1 </math> and <math> \mathbf {H}_2 </math> we get:
<math display="block">\mathbf {H}_2 \cdot (\nabla\times\mathbf {E}_1)-\mathbf {E}_1\cdot(\nabla\times\mathbf {H}_2) = \nabla\cdot(\mathbf {E}_1 \times\mathbf {H}_2)\ .</math>

If products in the Time-Periodic equations are taken as indicated by this last equivalence, and added,
<math display="block"> -\mathbf{H}_2\cdot j\omega \mathbf{B}_1 - \mathbf{E}_1 \cdot j\omega \mathbf{D}_2 - \mathbf{E}_1 \cdot \mathbf{J}_2 = \nabla \cdot(\mathbf{E}_1 \times \mathbf{H}_2)\ .</math>

This now may be integrated over the volume of concern,
<math display="block">\int_V \left(\mathbf{H}_2 \cdot j \omega \mathbf{B}_1+\mathbf{E}_1 \cdot j\omega \mathbf{D}_2+\mathbf{E}_1\mathbf{J}_2\right) \mathrm{d}V = -\int_V \nabla \cdot (\mathbf{E}_1 \times \mathbf{H}_2) \mathrm{d}V\ .</math> 

From the divergence theorem the volume integral of <math> \operatorname{div}(\mathbf{E}_1\times\mathbf{H}_2) </math> equals the surface integral of <math> \mathbf{E}_1\times\mathbf{H}_2 </math> over the boundary.
<math display="block">\int_V \left(\mathbf{H}_2 \cdot j\omega\mathbf{B}_1+\mathbf{E}_1\cdot j\omega\mathbf{D}_2+\mathbf{E}_1\cdot\mathbf{J}_2\right) \mathrm{d}V = -\oint_S(\mathbf{E}_1 \times \mathbf{H}_2)\cdot \widehat{\mathrm{d}S}\ .</math> 

This form is valid for general media, but in the common case of linear, isotropic, time-invariant materials, {{mvar|ε}} is a scalar independent of time. Then generally as physical magnitudes <math> \mathbf D = \epsilon\mathbf E </math> and <math> \mathbf B = \mu \mathbf H\ .</math>

Last equation then becomes
<math display="block">\int_V \left(\mathbf{H}_2 \cdot j \omega\mu\mathbf{H}_1+\mathbf{E}_1 \cdot j \omega \epsilon\mathbf{E}_2 + \mathbf{E}_1 \cdot \mathbf{J}_2\right) \mathrm{d}V = -\oint_S(\mathbf{E}_1\times\mathbf{H}_2) \cdot \widehat{\mathrm{d}S}\ .</math> 

In an exactly analogous way we get for vectors <math>\mathbf{E}_2</math> and <math>\mathbf{H}_1</math> the following expression:
<math display="block">\int_V \left(\mathbf{H}_1 \cdot j \omega \mu \mathbf{H}_2+\mathbf{E}_2 \cdot j \omega \epsilon\mathbf{E}_1 + \mathbf{E}_2 \cdot \mathbf{J}_1\right) \operatorname{d}V = -\oint_S(\mathbf{E}_2\times\mathbf{H}_1) \cdot \widehat{\mathrm{d}S}\ .</math> 

Subtracting the two last equations by members we get
<math display="block">\int_V \left[ \mathbf{J}_1 \cdot \mathbf{E}_2 - \mathbf{E}_1 \cdot \mathbf{J}_2 \right] \operatorname{d}V = \oint_S \left[ \mathbf{E}_1 \times \mathbf{H}_2 - \mathbf{E}_2 \times \mathbf{H}_1 \right] \cdot \mathbf{\mathrm{d}S}\ .</math>
and equivalently in differential form 
<math display="block">\ \mathbf{J}_1 \cdot \mathbf{E}_2 - \mathbf{E}_1 \cdot \mathbf{J}_2 = \nabla \cdot \left[ \mathbf{E}_1 \times \mathbf{H}_2 - \mathbf{E}_2 \times \mathbf{H}_1 \right]\ </math> [[Q.E.D.]] 

===Surface-term cancellation===
The cancellation of the surface terms on the right-hand side of the Lorentz reciprocity theorem, for an integration over all space, is not entirely obvious but can be derived in a number of ways. A rigorous treatment of the surface integral takes into account the [[causality]] of interacting wave field states: The surface-integral contribution at infinity vanishes for the time-convolution interaction of two causal wave fields only (the time-correlation interaction leads to a non-zero contribution).<ref>
{{cite book
 |author=Stumpf, M.
 |year=2018
 |title=Electromagnetic Reciprocity in Antenna Theory
 |publisher=IEEE Press / Wiley
 |at=§1.4.3
}}</ref> 

Another simple argument would be that the fields goes to zero at infinity for a localized source, but this argument fails in the case of lossless media: in the absence of absorption, radiated fields decay inversely with distance, but the surface area of the integral increases with the square of distance, so the two rates balance one another in the integral.

Instead, it is common (e.g. King, 1963) to assume that the medium is homogeneous and isotropic sufficiently far away. In this case, the radiated field asymptotically takes the form of [[planewave]]s propagating radially outward (in the <math> \operatorname{\hat{O}}{\mathbf{r}} </math> direction) with <math> \operatorname{\hat{O}}{\mathbf{r}} \cdot \mathbf{E} = 0 </math> and <math> \mathbf{H} = \hat{\mathbf{r}} \times \mathbf{E} / Z </math> where {{mvar|Z}} is the scalar [[Electrical impedance|impedance]] <math display="inline"> \sqrt{ \mu / \epsilon}</math> of the surrounding medium. Then it follows that <math>\ \mathbf{E}_1 \times \mathbf{H}_2 = \frac{ \mathbf{E}_1 \times \hat{\mathbf{r}} \times \mathbf{E}_2 }{Z}\ ,</math> which by a simple [[Cross product#Triple product expansion|vector identity]] equals <math> \frac{ \mathbf{E}_1 \cdot \mathbf{E}_2}{Z}\ \hat{\mathbf{r}}\ .</math> Similarly, <math> \mathbf{E}_2 \times \mathbf{H}_1 =  \frac{ \mathbf{E}_2 \cdot \mathbf{E}_1 }{Z} \ \hat{\mathbf{r}} </math> and the two terms cancel one another.

The above argument shows explicitly why the surface terms can cancel, but lacks generality. Alternatively, one can treat the case of lossless surrounding media with radiation boundary conditions imposed via the [[limiting absorption principle]] (LAP): Taking the limit as the losses (the imaginary part of {{mvar|ε}}) go to zero. For any nonzero loss, the fields decay exponentially with distance and the surface integral vanishes, regardless of whether the medium is homogeneous. Since the left-hand side of the Lorentz reciprocity theorem vanishes for integration over all space with any non-zero losses, it must also vanish in the limit as the losses go to zero. (Note that the LAP implicitly imposes the [[Sommerfeld radiation condition]] of zero incoming waves from infinity, because otherwise even an arbitrarily small loss would eliminate the incoming waves and the limit would not give the lossless solution.)

===Reciprocity and Green's function===
The inverse of the operator <math> \operatorname{\hat{O}}\ ,</math> i.e., in <math> \mathbf{E} = \operatorname{\hat{O}}^{-1} \mathbf{J} </math> (which requires a specification of the boundary conditions at infinity in a lossless system), has the same symmetry as <math> \operatorname{\hat{O}} </math> and is essentially a [[Green's function]] [[convolution]].  So, another perspective on Lorentz reciprocity is that it reflects the fact that convolution with the electromagnetic Green's function is a complex-symmetric (or anti-Hermitian, below) linear operation under the appropriate conditions on {{mvar|ε}} and {{mvar|μ}}. More specifically, the Green's function can be written as <math> G_{nm}(\mathbf{x}',\mathbf{x}) </math> giving the {{mvar|n}}-th component of <math> \mathbf{E} </math> at <math> \mathbf{x}' </math> from a point dipole current in the {{mvar|m}}-th direction at <math> \mathbf{x} </math> (essentially, <math> G </math> gives the matrix elements of <math> \operatorname{\hat{O}}^{-1} </math>), and Rayleigh-Carson reciprocity is equivalent to the statement that <math> G_{nm}(\mathbf{x}',\mathbf{x}) = G_{mn}(\mathbf{x},\mathbf{x}')\ .</math> Unlike <math> \operatorname{\hat{O}}\ ,</math> it is not generally possible to give an explicit formula for the Green's function (except in special cases such as homogeneous media), but it is routinely computed by numerical methods.

===Lossless magneto-optic materials===
One case in which {{mvar|ε}} is ''not'' a symmetric matrix is for [[magneto-optic]] materials, in which case the usual statement of Lorentz reciprocity does not hold (see below for a generalization, however). If we allow magneto-optic materials, but restrict ourselves to the situation where material ''absorption is negligible'', then {{mvar|ε}} and {{mvar|μ}} are in general 3×3 complex [[Hermitian matrices]]. In this case, the operator <math display="inline">\ \frac{1}{\mu} \left(\nabla \times \nabla \times\right) - \frac{\omega^2}{c^2} \varepsilon </math> is Hermitian under the ''conjugated'' inner product <math display="inline"> (\mathbf{F}, \mathbf{G}) = \int \mathbf{F}^* \cdot \mathbf{G} \, \mathrm{d}V\ ,</math> and a variant of the reciprocity theorem{{citation needed|date=October 2014}} still holds:
<math display="block"> - \int_V \left[ \mathbf{J}_1^* \cdot \mathbf{E}_2 + \mathbf{E}_1^* \cdot \mathbf{J}_2 \right] \mathrm{d}V = \oint_S \left[ \mathbf{E}_1^* \times \mathbf{H}_2 + \mathbf{E}_2 \times \mathbf{H}_1^* \right] \cdot \mathbf{\mathrm{d}A} </math>
where the sign changes come from the <math> \frac{1}{i\omega} </math> in the equation above, which makes the operator <math> \operatorname{\hat{O}} </math> [[anti-Hermitian]] (neglecting surface terms).  For the special case of <math> \mathbf{J}_1 = \mathbf{J}_2\ ,</math> this gives a re-statement of [[conservation of energy]] or [[Poynting's theorem]] (since here we have assumed lossless materials, unlike above): The time-average rate of work done by the current (given by the real part of <math> - \mathbf{J}^* \cdot \mathbf{E} </math>) is equal to the time-average outward flux of power (the integral of the [[Poynting vector]]). By the same token, however, the surface terms do not in general vanish if one integrates over all space for this reciprocity variant, so a Rayleigh-Carson form does not hold without additional assumptions.

The fact that magneto-optic materials break Rayleigh-Carson reciprocity is the key to devices such as [[Faraday isolator]]s and [[circulator]]s. A current on one side of a Faraday isolator produces a field on the other side but ''not'' vice versa.

===Generalization to non-symmetric materials===
For a combination of lossy and magneto-optic materials, and in general when the ε and μ tensors are neither symmetric nor Hermitian matrices, one can still obtain a generalized version of Lorentz reciprocity by considering <math> (\mathbf{J}_1, \mathbf{E}_1) </math> and <math> (\mathbf{J}_2, \mathbf{E}_2) </math> to exist in ''different systems''.

In particular, if <math> (\mathbf{J}_1, \mathbf{E}_1) </math> satisfy Maxwell's equations at ω for a system with materials <math> (\varepsilon_1, \mu_1)\ ,</math> and <math> (\mathbf{J}_2, \mathbf{E}_2) </math> satisfy Maxwell's equations at {{mvar|ω}} for a system with materials <math> \left(\varepsilon_1^\mathsf{T}, \mu_1^\mathsf{T} \right)\ ,</math> where <math> {}^\mathsf{T} </math> denotes the [[transpose]], then the equation of Lorentz reciprocity holds. This can be further generalized to [[bi-anisotropic material]]s by transposing the full 6×6 susceptibility tensor.<ref>
{{cite journal
 |first=Jin Au |last=Kong
 |year=1972 |title=Theorems of bianisotropic media
 |journal=Proceedings of the IEEE
 |volume=60 |number=9 |pages=1036–1046
 |doi=10.1109/PROC.1972.8851
}}</ref>

===Exceptions to reciprocity===
For [[nonlinear optics|nonlinear media]], no reciprocity theorem generally holds.  Reciprocity also does not generally apply for time-varying ("active") media; for example, when {{mvar|ε}} is modulated in time by some external process. (In both of these cases, the frequency {{mvar|ω}} is not generally a conserved quantity.)

==Feld-Tai reciprocity==
In 1992, a closely related reciprocity theorem was articulated independently by Y.A. Feld<ref name=Feld-1992>
{{cite journal
 |first=Ya.N. |last=Feld
 |year=1992
 |title=On the quadratic lemma in electrodynamics
 |journal=Sov. Phys. Dokl.
 |volume=37 |pages=235–236
}}
</ref> and C.T. Tai,<ref name=Tai-1992>
{{cite journal
 |first=C.-T. |last=Tai
 |year=1992
 |title=Complementary reciprocity theorems in electromagnetic theory
 |journal=IEEE Transactions on Antennas and Propagation
 |volume=40 |issue=6 |pages=675–681
|doi=10.1109/8.144602
 |bibcode=1992ITAP...40..675T
 |hdl=2027.42/21036
 |hdl-access=free
 }}
</ref>
and is known as '''Feld-Tai reciprocity''' or the '''Feld-Tai lemma'''. t relates two time-harmonic localized current sources and the resulting [[magnetic field]]s:

:<math>\int \mathbf{J}_1 \cdot \mathbf{H}_2 \, \operatorname{d}V = \int \mathbf{H}_1 \cdot \mathbf{J}_2 \, \operatorname{d}V\ .</math>

However, the Feld-Tai lemma is only valid under much more restrictive conditions than Lorentz reciprocity. It generally requires time-invariant linear media with an isotropic homogeneous [[Electrical impedance|impedance]], i.e. a constant [[scalar (physics)|scalar]] {{mvar|μ}}''/''{{mvar|ε}} ratio, with the possible exception of regions of perfectly conducting material.

More precisely, Feld-Tai reciprocity requires the Hermitian (or rather, complex-symmetric) symmetry of the electromagnetic operators as above, but also relies on the assumption that the  operator relating <math>\ \mathbf{E}\ </math> and <math>\ i \omega \mathbf{J}\ </math> is a constant scalar multiple of the  operator relating <math>\ \mathbf{H}\ </math> and <math>\ \nabla\times (\mathbf{J}/\varepsilon)\ ,</math> which is true when {{mvar|ε}} is a constant scalar multiple of {{mvar|μ}} (the two operators generally differ by an interchange of {{mvar|ε}} and {{mvar|μ}}). As above, one can also construct a more general formulation for integrals over a finite volume.

==Optical reciprocity in radiometric terms==

Apart from quantal effects, classical theory covers near-, middle-, and far-field electric and magnetic phenomena with arbitrary time courses. Optics refers to far-field nearly-sinusoidal oscillatory electromagnetic effects. Instead of paired electric and magnetic variables, optics, including optical reciprocity, can be expressed in [[Polarization (waves)|polarization]]-paired radiometric variables, such as [[spectral radiance]], traditionally called [[Specific radiative intensity|specific intensity]].

In 1856, [[Hermann von Helmholtz]] wrote:

::"A ray of light proceeding from point {{math|''A''}} arrives at point {{math|''B''}} after suffering any number of refractions, reflections, &c. At point {{math|''A''}} let any two perpendicular planes {{math|''a''<sub>1</sub>}}, {{math|''a''<sub>2</sub>}} be taken in the direction of the ray; and let the vibrations of the ray be divided into two parts, one in each of these planes. Take like planes {{math|''b''<sub>1</sub>}}, {{math|''b''<sub>2</sub>}} in the ray at point {{math|''B''}}; then the following proposition may be demonstrated. If when the quantity of light {{math|''J''}} polarized in the plane {{math|''a''<sub>1</sub>}} proceeds from {{math|''A''}} in the direction of the given ray, that part {{math|''K''}} thereof of light polarized in {{math|''b''<sub>1</sub>}} arrives at {{math|''B''}}, then, conversely, if the quantity of light {{math|''J''}} polarized in {{math|''b''<sub>1</sub>}} proceeds from {{math|''B''}}, the same quantity of light {{math|''K''}} polarized in {{math|''a''<sub>1</sub>}} will arrive at {{math|''A''}}."<ref name="Helmholtz 1856">{{cite book |last=von Helmholtz |first=H. |author-link=Hermann von Helmholtz |year=1856 |title=Handbuch der physiologischen Optik |trans-title=Handbook of Physiological Optics |edition=1st |publisher=Leopold Voss |place=Leipzig |volume=1 |page=169 |postscript=;}} cited by Planck. English version quoted here based on {{cite journal |title=translation of Helmholtz |translator=Guthrie, F. |journal=[[Philosophical Magazine]] |series=Series&nbsp;4 |volume=20 |pages=2–21 |type=Second printing |year=1867 |url=http://vlp.mpiwg-berlin.mpg.de/library/data/lit39509/index_html?pn=181&ws=1.5}}</ref>

This is sometimes called the [[Helmholtz reciprocity]] (or reversion) principle.<ref>{{cite journal |author=Minnaert, M. |year=1941 |title=The reciprocity principle in lunar photometry |journal=[[The Astrophysical Journal]] |volume=93 |pages=403–410 |doi=10.1086/144279 |bibcode=1941ApJ....93..403M |url=http://adsabs.harvard.edu/abs/1941ApJ....93..403M}}</ref><ref>{{cite book |author=Chandrasekhar, S. |author-link=Subrahmanyan Chandrasekhar |year=1950 |title=Radiative Transfer |publisher=Oxford University Press |place=Oxford, UK |pages=20-21, 171-177, 182}}</ref><ref>{{cite journal |author=Tingwaldt, C.P. |year=1952 |title=Über das Helmholtzsche Reziprozitätsgesetz in der Optik |trans-title=On the Helmholtz law of reciprocity in optics |journal=Optik |volume=9 |issue=6 |pages=248–253}}</ref><ref>{{cite book |author=Levi, L. |year=1968 |title=Applied Optics: A guide to optical system design |publisher=Wiley |place=New York, NY |volume=1 |page=84}} (2&nbsp;vols.)</ref><ref name="C&P 1985">{{cite journal |author1=Clarke, F.J.J. |author2=Parry, D.J. |year=1985 |title=Helmholtz reciprocity: Its validity and application to reflectometry |journal=[[Lighting Research & Technology]] |volume=17 |issue=1 |pages=1–11 |doi=10.1177/14771535850170010301 |s2cid=123394330}}</ref><ref name="B&W 1999 p 423">{{cite book |author1=Born, M. |author2=Wolf, E. |year=1999 |title=[[Principles of Optics]]: Electromagnetic theory of propagation, interference and diffraction of light |edition=7th |publisher=Cambridge University Press |isbn=0-521-64222-1 |page=423}}</ref> When the wave propagates through a material acted upon by an applied magnetic field, reciprocity can be broken so this principle will not apply.<ref name="Helmholtz 1856"/> Similarly, when there are moving objects in the path of the ray, the principle may be entirely inapplicable. Historically, in 1849, [[Sir George Stokes, 1st Baronet|Sir George Stokes]] stated his optical reversion principle without attending to polarization.<ref name="Stokes 1849">{{cite journal |author=Stokes, G.G. |author-link=Sir George Stokes, 1st Baronet |year=1849 |title=On the perfect blackness of the central spot in Newton's rings, and on the verification of Fresnel's formulae for the intensities of reflected and refracted rays |journal=Cambridge and Dublin Mathematical Journal |series=new series |volume=4 |pages=1–14}}</ref><ref>{{cite journal |author=Mahan, A.I. |year=1943 |title=A mathematical proof of Stokes' reversibility principle |journal=[[Journal of the Optical Society of America]] |volume=33 |issue=11 |pages=621–626|doi=10.1364/JOSA.33.000621 }}</ref><ref>{{cite book |author=Lekner, J. |year=1987 |title=Theory of Reflection of Electromagnetic and Particle Waves |publisher=Martinus Nijhoff |place=Dordrecht |isbn=90-247-3418-5 |pages=33–37 |url=https://books.google.com/books?id=mCYl2BTrCokC&q=Lekner+ISBN+9024734185 |via=Google Books}}</ref>

Like the principles of thermodynamics, this principle is reliable enough to use as a check on the correct performance of experiments, in contrast with the usual situation in which the experiments are tests of a proposed law.<ref name="Rayleigh 1900 reciprocity">{{cite journal |author=Rayleigh, J.W. Strutt, baron |author-link=John William Strutt, 3rd Baron Rayleigh |year=1900 |title=On the law of reciprocity in diffuse reflection |journal=[[Philosophical Magazine]] |series=series&nbsp;5 |volume=49 |pages=324–325}}</ref><ref name="Hapke 1993 10C">{{cite book |author=Hapke, B. |year=1993 |title=Theory of Reflectance and Emittance Spectroscopy |publisher=Cambridge University Press |place=Cambridge UK |isbn=0-521-30789-9 |at=Section&nbsp;10C, pages&nbsp;263-264}}</ref>

The simplest statement of the principle is ''if I can see you, then you can see me''. The principle was used by [[Gustav Kirchhoff]] in his derivation of [[Kirchhoff's law of thermal radiation|his law of thermal radiation]] and by [[Max Planck]] in his analysis of [[Planck's law|his law of thermal radiation]].

For ray-tracing [[global illumination]] algorithms, incoming and outgoing light can be considered as reversals of each other, without affecting the [[bidirectional reflectance distribution function]] (BRDF) outcome.<ref name="Hapke 1993 10C"/>

==Green's reciprocity==
Whereas the above reciprocity theorems were for oscillating fields, '''Green's reciprocity''' is an analogous theorem for electrostatics with a fixed distribution of [[electric charge]] (Panofsky and Phillips, 1962).

In particular, let <math>\phi_1</math> denote the electric potential resulting from a total charge density <math>\rho_1</math>.  The electric potential satisfies [[Poisson's equation]], <math>-\nabla^2 \phi_1 = \rho_1 / \varepsilon_0</math>, where <math>\varepsilon_0</math> is the [[vacuum permittivity]].  Similarly, let <math>\phi_2</math> denote the electric potential resulting from a total charge density <math>\rho_2</math>, satisfying <math>-\nabla^2 \phi_2 = \rho_2 / \varepsilon_0</math>.  In both cases, we assume that the charge distributions are localized, so that the potentials can be chosen to go to zero at infinity.  Then, Green's reciprocity theorem states that, for integrals over all space:

:<math>\int \rho_1 \phi_2 dV = \int \rho_2 \phi_1 \operatorname{d}V\ .</math>

This theorem is easily proven from [[Green's second identity]]. Equivalently, it is the statement that
: <math>\int \phi_2 ( \nabla^2 \phi_1 ) dV = \int \phi_1 ( \nabla^2 \phi_2 ) \operatorname{d}V\ ,</math>
i.e. that <math>\nabla^2</math> is a Hermitian operator (as follows by integrating by parts twice).

==See also==
*[[Surface equivalence principle]]

==References==

* L. D. Landau and E. M. Lifshitz, ''Electrodynamics of Continuous Media'' (Addison-Wesley: Reading, MA, 1960). §89.
* [[Ronold W. P. King]], ''Fundamental Electromagnetic Theory'' (Dover: New York, 1963).   	§IV.21.
* C. Altman and K. Such, ''Reciprocity, Spatial Mapping and Time Reversal in Electromagnetics'' (Kluwer: Dordrecht, 1991).
* H. A. Lorentz, [https://www.lorentz.leidenuniv.nl/IL-publications/sources/Lorentz_KNAW_1895.pdf "The theorem of Poynting concerning the energy in the electromagnetic field and two general propositions concerning the propagation of light,"] ''Versl. Kon. Akad. Wet. Amst.'' '''4''', 176-187 (1895/96).
* R. J. Potton, "Reciprocity in optics," ''Reports on Progress in Physics'' '''67''', 717-754 (2004).  (A review article on the history of this topic.)
* J. R. Carson, [https://archive.org/stream/bell00systemtechniamervol3rich#page/392/mode/2up "A generalization of reciprocal theorem,"] ''Bell System Technical Journal'' '''3''' (3), 393-399 (1924).
* J. R. Carson, [https://archive.org/stream/bstj9-2-325#page/n0/mode/2up "The reciprocal energy theorem,"] ''ibid''. '''9''' (4), 325-331 (1930).
* Ya. N. Feld, "On the quadratic lemma in electrodynamics," ''Sov. Phys&mdash;Dokl.'' '''37''', 235-236 (1992).
* C.-T. Tai, "Complementary reciprocity theorems in electromagnetic theory," ''IEEE Trans. Antennas Prop.'' '''40''' (6), 675-681 (1992).
* Wolfgang K. H. Panofsky and Melba Phillips, ''Classical Electricity and Magnetism'' (Addison-Wesley: Reading, MA, 1962).
* M. Stumpf,  ''Electromagnetic Reciprocity in Antenna Theory'' (Wiley-IEEE Press: Piscataway, NJ: 2018).
* M. Stumpf, ''Time-Domain Electromagnetic Reciprocity in Antenna Modeling'' (Wiley-IEEE Press: Piscataway, NJ: 2020).
* V. S. Asadchy, M. S. Mirmoosa, A. Díaz-Rubio, S. Fan and S. A. Tretyakov, "Tutorial on Electromagnetic Nonreciprocity and its Origins," in ''Proceedings of the IEEE'', vol. 108, no. 10, pp. 1684-1727, Oct. 2020, [[doi:10.1109/JPROC.2020.3012381]].

==Citations==
{{reflist|25em}}

[[Category:Electromagnetism]]
[[Category:Circuit theorems]]