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| Static force fields are fields, such as a simple electric, magnetic or gravitational fields, that exist without excitations. The [[Perturbation theory (quantum mechanics)|most common approximation method]] that physicists use for [[Scattering theory|scattering calculations]] can be interpreted as static forces arising from the interactions between two bodies mediated by [[virtual particles]], particles that exist for only a short time determined by the [[uncertainty principle]]. The virtual particles, also known as [[force carriers]], are [[bosons]] with a particular type of boson associated with each type of field.<ref>{{cite book | author=A. Zee | title=Quantum Field Theory in a Nutshell| publisher= Princeton University| year=2003 | isbn=0-691-01019-6}} pp. 16-37</ref>
| | <br><br>The Native makes use of a back lock design. To me, the American model of the lock feels much smoother than its Japanese cousins. It has the same authoritative "swack" that the Japanese fashions have; it is only a bit smoother. As I've stated in different critiques of knives from this line, the again lock design is not as strong as other designs. It sacrifices somewhat strength for lots of weight. But in follow, this lock design is ok for daily carry. In case you are stressing the lock, then you should in all probability be utilizing a hard and fast blade.<br><br>Aliexpress is the most effective place to come back to seek out useful Maxam Pocket Knife evaluations You can read probably the most in-depth critiques, ratings and feedbacks from people who have bought and used them. We have actual client critiques of different types of Maxam Pocket Knife , including wood deal with knife critiques , work knife reviews and more. Our Maxam Pocket Knife reviews will show you [http://www.thefreedictionary.com/pocket+knife hunting knives for sale] how to make the perfect purchase. Although you determined what sort of finest pocket knife to purchase, however nonetheless a variety of elements should take into account. This includes components akin to blade dimension , the aim you are using it for, steel kind and and so forth.<br><br>It isn't that tough truly. Victorinox has been for many years the main company in the market for pocket knives and multi-tools. The Swiss Army Knives have a top quality design far superior to every factor else out there, they are manufactured with excellent materials to last, and they are again up by a lifetime warranty. So, the logic selection is to select from them. But, although you really can't go mistaken buying a Victorinox, plainly some fashions are higher than others. A small change is the dimensions of the ribbing on the rubberized handle. The Pro Knife has bigger ribbing than the unique Final Knife.<br><br>My only critique of this knife is personal in nature. For one, I have always most well-liked a blade with enamel. A partially micro-dented blade for easily cutting cord and other materials seems the extra versatile choice. Second, the polycarbonate handle seems like extra of an aesthetic afterthought than a purposeful addition and the handle wasn’t noticeably less comfy after removing [http://Thebestpocketknifereviews.com/best-swiss-army-knife-choosing-the-best-models/ best Swiss army Knives] it. I removed the purple deal with slab when after a month or so I found myself tightening it down and decided as a substitute to do away with the difficulty altogether. They said sufferers ought to be counseled on the relative advantages and harms, as well as the costs of every graft possibility.<br><br>The most typical lock fastened in all conventional pocket knives is the one that gives method when stress is applied on the blade. Springs are fitted within the pivot to resist stress [http://Www.Decodiams.com/forum/index.php?a=member&m=863522 that's generated] when the knife is used. To close the blade, all you need to do is press the unsharpened facet of the blade and the blade will come free and fold into the deal with. This is adequate for most people who make use of such knives Nonetheless, as time goes by, the energy of the spring weakens and the knife closes even when the individual doesn't want it to.<br><br>When looking for the perfect pocket knife , be sure you comply with these simple but bizarre tips or else you is likely to be in for a big shock. Pocket knives can fluctuate vastly by way of design and, for that reason, it is best to decide one primarily based in your meant usage. This information will walk you through what it is best to search for in a pocket knife in addition to the highest 10 pocket knives really useful by KnifeUp. The knife comes with a condor sheath that, for a pocket knife, is uncommon and value a great price by itself. The condor sheath suits MOLLE gear for military and legislation enforcement personnel.<br><br>Howdy each physique if you happen to discover out. Victorinox Swiss Military Traditional SD Pocket Knife (Blue),And need to [http://Luciddesign.Dothome.co.kr/xe/board_DZQS66/49815 purchase] a superb one you meet it in here “Victorinox Swiss Army Basic SD Pocket Knife (Blue)”, Now we have good value for products, In Our Web site You can learn evaluations from real customers and You'll be able to test Costs Comparision before you buy with easy you gained’t miss it. 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| The virtual-particle description of static forces is capable of identifying the spacial form of the forces, such as the inverse-square behavior in [[Newton's Universal Law of Gravitation]] and in [[Coulomb's Law]]. It is also able to predict whether the forces are attractive or repulsive for like bodies.
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| The [[path integral formulation]] is the natural language for describing force carriers. This article uses the path integral formulation to describe the force carriers for [[Spin (physics)|spin]] 0, 1, and 2 fields. [[Pion]]s, [[photon]]s, and [[graviton]]s fall into these respective categories.
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| As with any physical theory, there are limits to the validity of the virtual particle picture. The virtual-particle formulation is derived from a method known as [[perturbation theory]] which is an approximation assuming interactions are not too strong, and was intended for scattering problems, not bound states such as atoms. For the strong force binding [[quarks]] into [[nucleons]] at low energies, perturbation theory has never been shown to yield results in accord with experiments,<ref>[http://www.hep.phy.cam.ac.uk/theory/research/hadronic.html]</ref> thus, the validity of the "force-mediating particle" picture is questionable. Similarly, for [[bound states]] the method fails.<ref>[http://galileo.phys.virginia.edu/classes/752.mf1i.spring03/Time_Ind_PT.htm]</ref> In these cases the physical interpretation must be re-examined.
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| As an example the calculations of atomic structure in atomic physics or of molecular structure in quantum chemistry could not easily be repeated, if at all, using the "force-mediating particle" picture.
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| Additionally one should look critically at the recent CERN experiments in which evidence is adduced for the physical reality of the Higgs boson, which is a force-mediating particle. One should be careful not to make the logical error known as [[Reification (fallacy)|reification]], which confuses concept and reality.
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| The "force-mediating particle" picture (FMPP) is used because the classical two-body interaction (Coulomb's law for example), depending on six spatial dimensions, is incompatible with the Lorentz invariance of Dirac's equation. The use of the FMPP is unnecessary in nonrelativistic quantum mechanics, and Coulomb's law is used as given in atomic physics and quantum chemistry to calculate both bound and scattering states. A nonperturbative relativistic quantum theory, in which Lorentz invariance is preserved, is achievable by evaluating Coulomb's law as a 4-space interaction using the 3-space position vector of a reference electron obeying Dirac's equation and the quantum trajectory of a second electron which depends only on the scaled time ct. The quantum trajectory of each electron in an ensemble is inferred from the Dirac current for each electron by setting it equal to a velocity field times a quantum density, calculating a position field from the time integral of the velocity field, and finally calculating a quantum trajectory from the expectation value of the position field. The quantum trajectories are of course spin dependent, and the theory can be validated by checking that Pauli's Exclusion Principle is obeyed for a collection of fermions.
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| ==Classical forces== | |
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| The force exerted by one mass on another and the force exerted by one charge on another are strikingly similar. Both fall off as the square of the distance between the bodies. Both are proportional to the product of properties of the bodies, mass in the case of gravitation and charge in the case of electrostatics.
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| They also have a striking difference. Two masses attract each other, while two like charges repel each other.
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| In both cases, the bodies appear to act on each other over a distance. The concept of [[Field (physics)|field]] was invented to mediate the interaction among bodies thus eliminating the need for [[Action at a distance (physics)|action at a distance]]. The gravitational force is mediated by the [[gravitational field]] and the Coulomb force is mediated by the [[electromagnetic field]].
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| ===Gravitational force===
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| The [[Newton's law of universal gravitation|gravitational force]] on a mass <math> m </math> exerted by another mass <math> M </math> is | |
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| : <math>
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| | |
| \mathbf{F} =
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| - G {m M \over {r}^2} | |
| \, \mathbf{\hat{r}} =
| |
| m \mathbf{g} \left ( \mathbf{r} \right ),
| |
| </math>
| |
| where ''G'' is the [[gravitational constant]], r is the distance between the masses, and <math> \mathbf{\hat{r}} </math> is the [[unit vector]] from mass <math> M </math> to mass <math> m </math>.
| |
| | |
| The force can also be written
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| : <math>
| |
| | |
| \mathbf{F} =
| |
| m \mathbf{g} \left ( \mathbf{r} \right ),
| |
| </math>
| |
| | |
| where <math> \mathbf{g} \left ( \mathbf{r} \right ) </math> is the [[gravitational field]] described by the field equation
| |
| | |
| :<math>\nabla\cdot \mathbf{g} = -4\pi G\rho_m, </math>
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| where <math>\rho_m</math> is the [[density|mass density]] at each point in space.
| |
| | |
| ===Coulomb force===
| |
| | |
| The electrostatic [[Coulomb force]] on a charge <math> q </math> exerted by a charge <math> Q </math> is ([[SI units]]) | |
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| :<math>\mathbf{F} = {1 \over 4\pi\varepsilon_0}{q Q \over r^2}\mathbf{\hat{r}},</math>
| |
| | |
| where <math> \varepsilon_0 </math> is the [[vacuum permittivity]], <math>r</math> is the separation of the two charges, and <math>\mathbf{\hat{r}}</math> is a [[unit vector]] in the direction from charge <math> Q </math> to charge <math> q </math>.
| |
| | |
| The Coulomb force can also be written in terms of an [[electrostatic field]]: | |
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| :<math>\mathbf{F} = q \mathbf{E} \left ( \mathbf{r} \right ),</math>
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| | |
| where
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| | |
| :<math> \nabla \cdot \mathbf{E} = \frac { \rho_q } { \varepsilon _0 };</math>
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| | |
| <math>\rho_q</math> being the [[density|charge density]] at each point in space.
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| ==Virtual-particle exchange==
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| In perturbation theory, forces are generated by the exchange of [[virtual particles]]. The mechanics of virtual-particle exchange is best described with the [[path integral formulation]] of quantum mechanics. There are insights that can be obtained, however, without going into the machinery of path integrals, such as why classical gravitational and electrostatic forces fall off as the inverse square of the distance between bodies.
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| ===Path-integral formulation of virtual-particle exchange===
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| A virtual particle is created by a disturbance to the [[vacuum state]], and the virtual particle is destroyed when it is absorbed back into the vacuum state by another disturbance. The disturbances are imagined to be due to bodies that interact with the virtual particle field.
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| ====The probability amplitude====
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| The probability amplitude for the creation, propagation, and destruction of a virtual particle is given, in the [[path integral formulation]] by
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| :<math> Z \equiv
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| \langle 0 | \exp\left ( -i \hat H T \right ) |0 \rangle
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| = \exp\left ( -i E T \right )
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| = \int D\varphi \; \exp\left ( i \mathcal{S} [\varphi] \right )\;
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| = \exp\left ( i W \right )
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| </math>
| |
| | |
| where <math> \hat H </math> is the [[Hamiltonian operator]], <math> T </math> is elapsed time, <math> E </math> is the energy change due to the disturbance, <math> W = - E T </math> is the change in action due to the disturbance, <math> \varphi </math> is the field of the virtual particle, the integral is over all paths, and the classical [[Action (physics)|action]] is given by
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| :<math>\mathcal{S} [\varphi] = \int \mathrm{d}^4x\; {\mathcal{L} [\varphi (x)]\,} </math>
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| | |
| where <math> \mathcal{L} [\varphi (x)] </math> is the [[Lagrangian]] density. We are using [[natural units]], <math> \hbar = c = 1 </math>.
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| | |
| Here, the [[spacetime]] metric is given by
| |
| | |
| :<math>\eta_{\mu\nu} = \begin{pmatrix}
| |
| 1 & 0 & 0 & 0\\
| |
| 0 & -1 & 0 & 0\\
| |
| 0 & 0 & -1 & 0\\
| |
| 0 & 0 & 0 & -1
| |
| \end{pmatrix}
| |
| .</math> | |
| | |
| The path integral often can be converted to the form
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|
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| :<math> Z=
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| \int \exp\left[ i \int d^4x \left ( \frac 1 2 \varphi \hat O \varphi + J \varphi \right) \right ] D\varphi
| |
| </math>
| |
| | |
| where <math> \hat O </math> is a differential operator with <math> \varphi </math> and <math> J </math> functions of [[spacetime]]. The first term in the argument represents the free particle and the second term represents the disturbance to the field from an external source such as a charge or a mass.
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| The integral can be written (see [[Common integrals in quantum field theory#Integrals with differential operators in the argument|Common integrals in quantum field theory]])
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| :<math> Z \propto
| |
| \exp\left( i W\left ( J \right )\right)
| |
| </math>
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| | |
| where
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| | |
| :<math> W\left ( J \right ) =
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| -{1\over 2} \iint d^4x \; d^4y \; J\left ( x \right ) D\left ( x-y \right ) J\left ( y \right )
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| </math>
| |
| | |
| is the change in the action due to the disturbances and the [[propagator]] <math> D\left ( x-y \right ) </math> is the solution of | |
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| :<math>
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| \hat O D\left ( x - y \right ) = \delta^4 \left ( x - y \right )
| |
| </math>.
| |
| | |
| ====Energy of interaction====
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| | |
| We assume that there are two point disturbances representing two bodies and that the disturbances are motionless and constant in time. The disturbances can be written
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| :<math> J\left ( x \right )
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| = \left( J_1 +J_2,0,0,0 \right)
| |
| | |
| </math>
| |
| | |
| :<math> J_1 =
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| a_1 \delta^3\left ( \vec x - \vec x_1 \right )
| |
| | |
| </math>
| |
| | |
| :<math> J_2 =
| |
| a_2 \delta^3\left ( \vec x - \vec x_2 \right )
| |
| | |
| </math>
| |
| | |
| where the delta functions are in space, the disturbances are located at <math> \vec x_1 </math> and <math> \vec x_2 </math>, and the coefficients <math> a_1 </math> and <math> a_2 </math> are the strengths of the disturbances.
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| If we neglect self-interactions of the disturbances then W becomes
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| :<math> W\left ( J \right ) =
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| - \iint d^4x \; d^4y \; J_1\left ( x \right ) {1\over 2} \left [ D\left ( x-y \right ) + D\left ( y-x \right )\right ] J_2\left ( y \right )
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| </math>,
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| | |
| which can be written
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| | |
| :<math> W\left ( J \right ) =
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| - T a_1 a_2\int {d^3k \over (2 \pi )^3 } \; \; D\left ( k \right )\mid_{k_0=0} \; \exp\left ( i \vec k \cdot \left ( \vec x_1 - \vec x_2 \right ) \right )
| |
| </math>.
| |
| | |
| Here <math> D\left ( k \right ) </math> is the Fourier transform of
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| :<math> {1\over 2} \left [ D\left ( x-y \right ) + D\left ( y-x \right )\right ]
| |
| </math>.
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| Finally, the change in energy due to the static disturbances of the vacuum is
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| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
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| <math> E =
| |
| -{W\over T}=
| |
| a_1 a_2\int {d^3k \over (2 \pi )^3 } \; \; D\left ( k \right )\mid_{k_0=0} \; \exp\left ( i \vec k \cdot \left ( \vec x_1 - \vec x_2 \right ) \right )
| |
| </math>.
| |
| |}
| |
| | |
| If this quantity is negative, the force is attractive. If it is positive, the force is repulsive.
| |
| | |
| Examples of static, motionless, interacting currents are [[Static forces and virtual-particle exchange#The Yukawa potential: The force between two nucleons in an atomic nucleus|Yukawa Potential]], [[Static forces and virtual-particle exchange#The Coulomb potential in a vacuum|The Coulomb potential in a vacuum]], and [[Static forces and virtual-particle exchange#Coulomb potential in a simple plasma or electron gas|Coulomb potential in a simple plasma or electron gas]].
| |
| | |
| The expression for the interaction energy can be generalized to the situation in which the point particles are moving, but the motion is slow compared with the speed of light. Examples are [[Static forces and virtual-particle exchange#Darwin interaction in a vacuum|Darwin interaction in a vacuum]] and [[Static forces and virtual-particle exchange#Darwin interaction in a plasma|Darwin interaction in a plasma]].
| |
| | |
| Finally, the expression for the interaction energy can be generalized to situations in which the disturbances are not point particles, but are possibly line charges, tubes of charges, or current vortices. Examples are [[Static forces and virtual-particle exchange#Two line charges embedded in a plasma or electron gas|Two line charges embedded in a plasma or electron gas]], [[Static forces and virtual-particle exchange#Coulomb potential between two current loops embedded in a magnetic field|Coulomb potential between two current loops embedded in a magnetic field]], and [[Static forces and virtual-particle exchange#Magnetic interaction between current loops in a simple plasma or electron gas|Magnetic interaction between current loops in a simple plasma or electron gas]]. As seen from the Coulomb interaction between tubes of charge example, these more complicated geometries can lead to such exotic phenomena as [[Fractional quantum Hall effect|fractional quantum numbers]].
| |
| | |
| ==Selected examples==
| |
| | |
| ===The Yukawa potential: The force between two nucleons in an atomic nucleus===
| |
| | |
| Consider the [[Spin (physics)|spin]]-0 Lagrangian density<ref>Zee, pp. 21-29</ref>
| |
| | |
| :<math>
| |
| \mathcal{L} [\varphi (x)]
| |
| = {1\over 2} \left [ \left ( \partial \varphi \right )^2 -m^2 \varphi^2 \right ]
| |
| </math>.
| |
| | |
| The equation of motion for this Lagrangian is the [[Klein-Gordon equation]]
| |
| | |
| :<math>
| |
| \partial^2 \varphi + m^2 \varphi =0
| |
| </math>.
| |
| | |
| If we add a disturbance the probability amplitude becomes
| |
| | |
| :<math>
| |
| Z =
| |
| \int D\varphi \; \exp \left \{ i \int d^4x\; \left [ {1\over 2} \left ( \left ( \partial \varphi \right )^2 - m^2\varphi^2 \right ) + J\varphi \right ] \right \}
| |
| </math>.
| |
| | |
| If we integrate by parts and neglect boundary terms at infinity the probability amplitude becomes
| |
| | |
| :<math>
| |
| Z =
| |
| \int D\varphi \; \exp \left \{ i \int d^4x\; \left [ -{1\over 2}\varphi \left ( \partial^2 + m^2\right )\varphi + J\varphi \right ] \right \}
| |
| </math>.
| |
| | |
| With the amplitude in this form it can be seen that the propagator is the solution of
| |
| | |
| :<math>
| |
| -\left ( \partial^2 + m^2\right ) D\left ( x-y \right ) = \delta^4\left ( x-y \right )
| |
| </math>.
| |
| | |
| From this it can be seen that
| |
| | |
| :<math>
| |
| D\left ( k \right )\mid_{k_0=0}\; = \;
| |
| -{1 \over \vec k^2 + m^2}
| |
| </math>.
| |
| | |
| The energy due to the static disturbances becomes (see [[Common integrals in quantum field theory#Yukawa Potential: The Coulomb potential with mass|Common integrals in quantum field theory]])
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E =
| |
| -{a_1 a_2 \over 4 \pi r } \exp \left ( -m r \right )
| |
| </math>
| |
| |}
| |
| | |
| with
| |
| | |
| :<math>
| |
| r^2 =
| |
| \left (\vec x_1 - \vec x_2 \right )^2
| |
| </math>
| |
| | |
| which is attractive and has a range of
| |
| | |
| :<math>
| |
| {1 \over m}
| |
| </math>.
| |
| | |
| [[Yukawa]] proposed that this field describes the force between two [[nucleon]]s in an atomic nucleus. It allowed him to predict both the range and the mass of the particle, now known as the [[pion]], associated with this field.
| |
| | |
| ===Electrostatics===
| |
| | |
| ====The Coulomb potential in a vacuum====
| |
| | |
| Consider the [[Spin (physics)|spin]]-1 [[Proca action|Proca Lagrangian]] with a disturbance<ref>Zee, pp. 30-31</ref>
| |
| | |
| :<math>
| |
| \mathcal{L} [\varphi (x)] =
| |
| -{1\over 4} F_{\mu \nu} F^{\mu \nu} + {1\over 2} m^2 A_{\mu} A^{\mu} + A_{\mu} J^{\mu}
| |
| </math>
| |
| | |
| where
| |
| | |
| :<math>
| |
| F_{\mu \nu} =
| |
| \partial_{\mu} A_{\nu} - \partial_{\nu} A_{\mu}
| |
| </math>,
| |
| | |
| charge is conserved
| |
| | |
| :<math>
| |
| \partial_{\mu} J^{\mu} = 0
| |
| </math>,
| |
| | |
| and we choose the [[Lorenz gauge]]
| |
| | |
| :<math>
| |
| \partial_{\mu} A^{\mu} = 0
| |
| </math>.
| |
| | |
| Moreover, we assume that there is only a time-like component <math>J^{0} </math> to the disturbance. In ordinary language, this means that there is a charge at the points of disturbance, but there are no electric currents.
| |
| | |
| If we follow the same procedure as we did with the Yukawa potential we find that
| |
| | |
| :<math>
| |
| -{1\over 4} \int d^4x F_{\mu \nu}F^{\mu \nu}
| |
| = -{1\over 4}\int d^4x \left( \partial_{\mu} A_{\nu} - \partial_{\nu} A_{\mu} \right)\left( \partial^{\mu} A^{\nu} - \partial^{\nu} A^{\mu} \right)
| |
| </math>
| |
| | |
| :<math>
| |
| = {1\over 2}\int d^4x \; A_{\nu} \left( \partial^{2} A^{\nu} - \partial^{\nu} \partial_{\mu} A^{\mu} \right)
| |
| = {1\over 2}\int d^4x \; A^{\mu} \left( \eta_{\mu \nu} \partial^{2} \right) A^{\nu}
| |
| ,</math>
| |
| | |
| which implies
| |
| | |
| :<math>
| |
| \eta_{\mu \alpha} \left ( \partial^2 + m^2\right ) D^{\alpha \nu}\left ( x-y \right ) = \delta_{\mu }^{ \nu} \delta^4\left ( x-y \right )
| |
| </math>
| |
| | |
| and
| |
| | |
| :<math>
| |
| D_{\mu \nu}\left ( k \right )\mid_{k_0=0}\; = \;
| |
| \eta_{\mu \nu}{1 \over - k^2 + m^2}
| |
| .</math>
| |
| | |
| This yields
| |
| | |
| :<math>
| |
| D\left ( k \right )\mid_{k_0=0}\; = \;
| |
| {1 \over \vec k^2 + m^2}
| |
| </math>
| |
| | |
| for the [[timelike]] propagator and
| |
| | |
| :<math>
| |
| E =
| |
| {a_1 a_2 \over 4 \pi r } \exp \left ( -m r \right )
| |
| </math>
| |
| | |
| which has the opposite sign to the Yukawa case.
| |
| | |
| In the limit of zero [[photon]] mass, the Lagrangian reduces to the Lagrangian for [[electromagnetism]]
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E =
| |
| {a_1 a_2 \over 4 \pi r }
| |
| .</math>
| |
| |}
| |
| | |
| Therefore the energy reduces to the potential energy for the Coulomb force and the coefficients <math>a_1 </math> and <math>a_2 </math> are proportional to the electric charge. Unlike the Yukawa case, like bodies, in this electrostatic case, repel each other.
| |
| | |
| ====Coulomb potential in a simple plasma or electron gas====
| |
| | |
| =====Plasma waves=====
| |
| | |
| The [[dispersion relation]] for [[plasma wave]]s is<ref>{{cite book | author=F. F. Chen | title=Introduction to Plasma Physics| publisher= Plenum Press| year=1974 | isbn=0-306-30755-3}} pp. 75-82</ref>
| |
| | |
| :<math>
| |
| \omega^2 = \omega_p^2 + \gamma\left( \omega \right) {T_e\over m} \vec k^2
| |
| .</math>
| |
| | |
| where <math>\omega </math> is the angular frequency of the wave,
| |
| | |
| :<math>
| |
| \omega_p^2 = {4\pi n e^2 \over m}
| |
| </math>
| |
| | |
| is the [[plasma frequency]], <math>e </math> is the magnitude of the [[electron charge]], <math>m </math> is the [[electron mass]], <math>T_e </math> is the electron [[temperature]] ([[Boltzmann's constant]] equal to one), and <math>\gamma\left( \omega \right) </math> is a factor that varies with frequency from one to three. At high frequencies, on the order of the plasma frequency, the compression of the electron fluid is an [[adiabatic process]] and <math>\gamma\left( \omega \right) </math> is equal to three. At low frequencies, the compression is an [[isothermal process]] and <math>\gamma\left( \omega \right) </math> is equal to one. [[Retarded potential|Retardation]] effects have been neglected in obtaining the plasma-wave dispersion relation.
| |
| | |
| For low frequencies, the dispersion relation becomes
| |
| | |
| :<math>
| |
| \vec k^2 + \vec k_D^2
| |
| =0
| |
| </math>
| |
| | |
| where
| |
| | |
| :<math>
| |
| k_D^2
| |
| = {4\pi n e^2 \over T_e}
| |
| </math>
| |
| | |
| is the Debye number, which is the inverse of the [[Debye length]]. This suggests that the propagator is
| |
| | |
| :<math>
| |
| D\left ( k \right )\mid_{k_0=0}\; = \;
| |
| {1 \over \vec k^2 + k_D^2}
| |
| </math>.
| |
| | |
| In fact, if the retardation effects are not neglected, then the dispersion relation is
| |
| | |
| :<math>
| |
| -k_0^2 +\vec k^2 + k_D^2 -{m \over T_e} k_0^2
| |
| =0
| |
| ,</math>
| |
| | |
| which does indeed yield the guessed propagator. This propagator is the same as the massive Coulomb propagator with the mass equal to the inverse Debye length. The interaction energy is therefore
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E =
| |
| {a_1 a_2 \over 4 \pi r } \exp \left ( -k_D r \right )
| |
| .</math>
| |
| |}
| |
| The Coulomb potential is screened on length scales of a Debye length.
| |
| | |
| =====Plasmons=====
| |
| | |
| In a quantum [[electron gas]], plasma waves are known as [[plasmons]]. Debye screening is replaced with [[Thomas-Fermi screening]] to yield<ref>{{cite book | author=C. Kittel | title=Introduction to Solid State Physics, Fifth Edition| publisher= John Wiley and Sons| year=1976 | isbn=0-471-49024-5}} pp. 296-299.</ref>
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E =
| |
| {a_1 a_2 \over 4 \pi r } \exp \left ( -k_s r \right )
| |
| </math>
| |
| |}
| |
| | |
| where the inverse of the Thomas-Fermi screening length is
| |
| | |
| :<math>
| |
| k_s^2
| |
| = {6\pi n e^2 \over \epsilon_F}
| |
| </math>
| |
| | |
| and <math>\epsilon_F</math> is the [[Fermi energy]]
| |
| | |
| <math>\epsilon_F = \frac{\hbar^2}{2m} \left( {3 \pi^2 n} \right)^{2/3} \,.</math>
| |
| | |
| This expression can be derived from the [[chemical potential]] for an [[electron gas]] and from [[Poisson's equation]]. The chemical potential for an electron gas near equilibrium is constant and given by
| |
| | |
| :<math>
| |
| \mu =
| |
| -e\varphi + \epsilon_F
| |
| </math>
| |
| | |
| where <math>\varphi</math> is the [[electric potential]]. Linearizing the Fermi energy to first order in the density fluctuation and combining with Poisson's equation yields the screening length. The force carrier is the quantum version of the [[plasma wave]].
| |
| | |
| =====Two line charges embedded in a plasma or electron gas=====
| |
| | |
| We consider a line of charge with axis in the z direction embedded in an [[electron gas]]
| |
| | |
| :<math>
| |
| J_1\left( x\right)
| |
| =
| |
| {a_1 \over L_B} {1 \over 2 \pi r} \delta^2\left( r \right)
| |
| </math>
| |
| | |
| where <math>r</math> is the distance in the xy plane from the line of charge, <math>L_B</math> is the width of the material in the z direction. The superscript 2 indicates that the [[Dirac delta function]] is in two dimensions. The propagator is
| |
| | |
| :<math>
| |
| D\left ( k \right )\mid_{k_0=0}\; = \;
| |
| {1 \over \vec k^2 + k_{Ds}^2}
| |
| </math>
| |
| | |
| where <math>k_{Ds} </math> is either the inverse [[Debye–Hückel equation|Debye-Hückel screening length]] or the inverse [[Thomas-Fermi screening]] length.
| |
| | |
| The interaction energy is
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| :<math>
| |
| E=
| |
| \left( { a_1\, a_2 \over 2 \pi L_B}\right) \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + k_{Ds}^2 }
| |
| \mathcal J_0 \left ( kr_{12} \right)
| |
| = \left( { a_1\, a_2 \over 2 \pi L_B}\right) K_0 \left( k_{Ds} r_{12} \right)
| |
| </math>
| |
| |}
| |
| | |
| where
| |
| | |
| :<math>
| |
| \mathcal J_n \left ( x \right)
| |
| </math>
| |
| | |
| and
| |
| | |
| :<math>
| |
| K_0 \left ( x \right)
| |
| </math>
| |
| | |
| are [[Bessel function]]s and <math> r_{12}</math> is the distance between the two line charges. In obtaining the interaction energy we made use of the integrals (see [[Common integrals in quantum field theory#Integration of the cylindrical propagator with mass|Common integrals in quantum field theory]])
| |
| | |
| :<math>
| |
| \int_0^{2 \pi} {d\varphi \over 2 \pi} \exp\left( i p \cos\left( \varphi \right) \right)
| |
| =
| |
| \mathcal J_0 \left( p \right)
| |
| </math>
| |
| | |
| and
| |
| | |
| :<math>
| |
| \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + m^2 }
| |
| \mathcal J_0 \left ( kr \right)
| |
| = K_0 \left( m r \right)
| |
| .</math>
| |
| | |
| For <math> k_{Ds} r_{12} << 1</math>, we have
| |
| | |
| :<math>
| |
| K_0 \left( k_{Ds} r_{12} \right) \rightarrow -\ln \left( {k_{Ds} r_{12} \over 2}\right) + 0.5772
| |
| .</math>
| |
| | |
| ====Coulomb potential between two current loops embedded in a magnetic field====
| |
| | |
| =====Interaction energy for vortices=====
| |
| | |
| We consider a charge density in tube with axis along a magnetic field embedded in an [[electron gas]]
| |
| | |
| :<math>
| |
| J_1\left( x\right)
| |
| =
| |
| {a_1 \over L_b} {1 \over 2 \pi r} \delta^2\left( r - r_{B1}\right)
| |
| </math>
| |
| | |
| where <math>r</math> is the distance from the [[guiding center]], <math>L_B</math> is the width of the material in the direction of the magnetic field
| |
| | |
| :<math>
| |
| r_{B1}
| |
| =
| |
| {\sqrt{4 \pi}m_1v_1\over a_1 B}
| |
| =
| |
| \sqrt { 2 \hbar \over m_1 \omega_c }
| |
| </math>
| |
| | |
| where the [[cyclotron frequency]] is ([[Gaussian units]])
| |
| | |
| :<math>
| |
| \omega_c =
| |
| { a_1 B \over \sqrt{4 \pi} m_1 c}
| |
| </math>
| |
| | |
| and
| |
| | |
| :<math>
| |
| v_{1}
| |
| =
| |
| \sqrt {2 \hbar \omega_c \over m_1}
| |
| </math>
| |
| | |
| is the speed of the particle about the magnetic field, and B is the magnitude of the magnetic field. The speed formula comes from setting the classical kinetic energy equal to the spacing between [[Landau levels]] in the quantum treatment of a charged particle in a magnetic field.
| |
| | |
| In this geometry, the interaction energy can be written
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| :<math>
| |
| E=
| |
| \left( { a_1\, a_2 \over 2 \pi L_B}\right) \int_0^{\infty} {k\;dk \;} D\left( k \right) \mid_{k_0=k_B=0}
| |
| \mathcal J_0 \left ( kr_{B1} \right) \mathcal J_0 \left ( kr_{B2} \right) \mathcal J_0 \left ( kr_{12} \right)
| |
| </math>
| |
| |}
| |
| | |
| where <math>r_{12}</math> is the distance between the centers of the current loops and
| |
| | |
| :<math>
| |
| \mathcal J_n \left ( x \right)
| |
| </math>
| |
| | |
| is a [[Bessel function]] of the first kind. In obtaining the interaction energy we made use of the integral
| |
| | |
| :<math>
| |
| \int_0^{2 \pi} {d\varphi \over 2 \pi} \exp\left( i p \cos\left( \varphi \right) \right)
| |
| =
| |
| \mathcal J_0 \left( p \right)
| |
| . </math>
| |
| | |
| =====Electric field due to a density perturbation=====
| |
| | |
| The [[chemical potential]] near equilibrium, is given by
| |
| | |
| :<math>
| |
| \mu =
| |
| -e\varphi + N\hbar \omega_c
| |
| =
| |
| N_0\hbar \omega_c
| |
| </math>
| |
| | |
| where <math>
| |
| -e\varphi
| |
| </math> is the [[potential energy]] of an electron in an [[electric potential]] and <math>
| |
| N_0
| |
| </math> and <math>
| |
| N
| |
| </math> are the number of particles in the [[electron gas]] in the absence of and in the presence of an electrostatic potential, respectively.
| |
| | |
| The density fluctuation is then
| |
| | |
| :<math>
| |
| \delta n =
| |
| {e \varphi \over \hbar \omega_c A_M L_B}
| |
| </math>
| |
| | |
| where <math>
| |
| A_M
| |
| </math> is the area of the material in the plane perpendicular to the magnetic field.
| |
| | |
| [[Poisson's equation]] yields
| |
| | |
| :<math>
| |
| \left( k^2 + k_B^2 \right) \varphi = 0
| |
| </math>
| |
| | |
| where
| |
| | |
| :<math>
| |
| k_B^2 = {4 \pi e^2 \over \hbar \omega_c A_M L_B}
| |
| .</math>
| |
| | |
| The propagator is then
| |
| | |
| :<math>
| |
| D\left( k \right) \mid_{k_0=k_B=0}
| |
| =
| |
| {1 \over
| |
| k^2 + k_B^2 }
| |
| | |
| </math>
| |
| | |
| and the interaction energy becomes
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| :<math>
| |
| E=
| |
| \left( { a_1\, a_2 \over 2 \pi L_B}\right) \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + k_B^2 }
| |
| \mathcal J_0 \left ( kr_{B1} \right) \mathcal J_0 \left ( kr_{B2} \right) \mathcal J_0 \left ( kr_{12} \right)
| |
| =
| |
| \left( { 2 e^2 \over L_B}\right) \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + k_B^2 r_B^2 }
| |
| \mathcal J_0^2 \left ( k \right) \mathcal J_0 \left ( k{r_{12}\over r_B} \right)
| |
| </math>
| |
| |}
| |
| | |
| where in the second equality ([[Gaussian units]]) we assume that the vortices had the same energy and the electron charge.
| |
| | |
| In analogy with [[plasmons]], the [[force carrier]] is the quantum version of the [[upper hybrid oscillation]] which is a longitudinal [[plasma wave]] that propagates perpendicular to the magnetic field.
| |
| | |
| =====Currents with angular momentum=====
| |
| | |
| ======Delta function currents======
| |
| | |
| [[Image:100927c Angular momentum 11.jpg|thumb|250px|right|Figure 1. Interaction energy vs. r for angular momentum states of value one. The curves are identical to these for any values of <math>{\mathit l}= {\mathit l^{\prime}}</math>. Lengths are in units are in <math>r_{\mathit l}</math>, and the energy is in units of <math>\left( { e^2 \over L_B}\right)</math>. Here <math>r = r_{12}</math>. Note that there are local minima for large values of <math> k_{B}</math>.]]
| |
| [[Image:100927 Angular momentum 15.jpg|thumb|250px|right|Figure 2. Interaction energy vs. r for angular momentum states of value one and five.]]
| |
| [[Image:101005 energy by theta.jpg|thumb|250px|right|Figure 3. Interaction energy vs. r for various values of theta. The lowest energy is for <math>\theta = {\pi\over 4 }</math> or <math> { \mathit l \over \mathit l^{\prime} } = 1 </math>. The highest energy plotted is for <math>\theta = 0.90{\pi\over 4 }</math>. Lengths are in units of <math>r_{\mathit l \mathit l^{\prime}}</math>.]]
| |
| [[Image:101011 energy picture.jpg|thumb|250px|right|Figure 4. Ground state energies for even and odd values of angular momenta. Energy is plotted on the vertical axis and r is plotted on the horizontal. When the total angular momentum is even, the energy minimum occurs when <math> { \mathit l = \mathit l^{\prime} } </math> or <math> { \mathit l \over \mathit l^{*} } = {1 \over 2} </math>. When the total angular momentum is odd, there are no integer values of angular momenta that will lie in the energy minimum. Therefore, there are two states that lie on either side of the minimum. Because <math> { \mathit l \ne \mathit l^{\prime} } </math>, the total energy is higher than the case when <math> { \mathit l = \mathit l^{\prime} } </math> for a given value of <math> { \mathit l^{*} } </math>.]]
| |
| Unlike classical currents, quantum current loops can have various values of the [[Larmor radius]] for a given energy.<ref>{{cite book | author=Z. F. Ezewa | title=Quantum Hall Effects, Second Edition| publisher= World Scientific| year=2008 | isbn=981-270-032-3}} pp. 187-190</ref> [[Landau level]]s, the energy states of a charged particle in the presence of a magnetic field, are multiply [[Degenerate energy level|degenerate]]. The current loops correspond to [[angular momentum]] states of the charged particle that may have the same energy. Specifically, the charge density is peaked around radii of
| |
| | |
| :<math>
| |
| r_{\mathit l} = \sqrt{\mathit l}\;r_B\; \; \; \mathit l=0,1,2, \ldots
| |
| </math>
| |
| | |
| where <math>\mathit l</math> is the angular momentum [[quantum number]]. When <math>\mathit l=1</math> we recover the classical situation in which the electron orbits the magnetic field at the [[Larmor radius]]. If currents of two angular momentum <math>\mathit l^{ }_{ }>0 </math> and <math>\mathit l^{\prime} \ge \mathit l^{ }_{ } </math> interact, and we assume the charge densities are delta functions at radius <math>r_{\mathit l}</math>, then the interaction energy is
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| :<math>
| |
| E=
| |
|
| |
| \left( { 2 e^2 \over L_B}\right) \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + k_B^2 r_{\mathit l}^2 }
| |
| \;\mathcal J_0 \left ( k \right) \;\mathcal J_0 \left ( \sqrt{{\mathit l^{\prime}}\over {\mathit l}} \;k \right) \;\mathcal J_0 \left ( k{r_{12}\over r_{\mathit l}} \right)
| |
| .</math>
| |
| |}
| |
| | |
| The interaction energy for <math>\mathit l=\mathit l^{\prime}</math> is given in Figure 1 for various values of <math>k_B r_{\mathit l}</math>. The energy for two different values is given in Figure 2.
| |
| | |
| ======Quasiparticles======
| |
| | |
| For large values of angular momentum, the energy can have local minima at distances other than zero and infinity. It can be numerically verified that the minima occur at
| |
| | |
| :<math>
| |
| r_{12}
| |
| =r_{\mathit l \mathit l^{\prime}}
| |
| = \sqrt{\mathit l + \mathit l^{\prime}}\;r_B
| |
| .</math>
| |
| | |
| This suggests that the pair of particles that are bound and separated by a distance <math>r_{\mathit l \mathit l^{\prime}} </math> act as a single [[quasiparticle]] with angular momentum <math> \mathit l + \mathit l^{\prime}</math>.
| |
| | |
| If we scale the lengths as <math> r_{\mathit l \mathit l^{\prime}} </math>, then the interaction energy becomes
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| :<math>
| |
| E=
| |
|
| |
| \left( { 2 e^2 \over L_B}\right) \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + k_B^2 r_{\mathit l \mathit l^{\prime}}^2 }
| |
| \;\mathcal J_0 \left ( \cos \theta \; k \right) \;\mathcal J_0 \left ( \sin \theta \;k \right) \;\mathcal J_0 \left ( k{r_{12}\over r_{\mathit l \mathit l^{\prime}}} \right)
| |
| </math>
| |
| |}
| |
| | |
| where
| |
| | |
| :<math>
| |
| \tan \theta
| |
| = \sqrt{\mathit l \over \mathit l^{\prime}}
| |
| .</math>
| |
| | |
| The value of the <math> r_{12} </math> at which the energy is minimum, <math>r_{12} = r_{\mathit l \mathit l^{\prime}} </math>, is independent of the ratio <math> \tan \theta = \sqrt{\mathit l \over \mathit l^{\prime}}</math>. However the value of the energy at the minimum depends on the ratio. The lowest energy minimum occurs when
| |
| | |
| : <math> {\mathit l \over \mathit l^{\prime}} = 1.</math>
| |
| | |
| When the ratio differs from 1, then the energy minimum is higher (Figure 3). Therefore, for even values of total momentum, the lowest energy occurs when (Figure 4)
| |
| | |
| : <math> \mathit l = \mathit l^{\prime} = 1</math>
| |
| | |
| or
| |
| | |
| : <math> {\mathit l \over \mathit l^*} = {1 \over 2} </math>
| |
| | |
| where the total angular momentum is written as
| |
| | |
| : <math> { \mathit l^*} = { \mathit l} + { \mathit l^{\prime} }. </math>
| |
| | |
| When the total angular momentum is odd, the minima cannot occur for <math> {\mathit l = \mathit l^{\prime}} . </math> The lowest energy states for odd total angular momentum occur when
| |
| | |
| : <math> {\mathit l \over \mathit l^*} = \; {\mathit l^*\pm 1 \over 2 \mathit l^* }</math>
| |
| | |
| or
| |
| | |
| :<math>{\mathit l \over \mathit l^*} ={1\over 3}, {2\over 5}, {3\over 7}, \mbox{etc.,} </math>
| |
| | |
| and
| |
| | |
| :<math>{\mathit l \over \mathit l^*} ={2\over3}, {3\over 5}, {4\over 7}, \mbox{etc.,} </math>
| |
| | |
| which also appear as series for the filling factor in the [[fractional quantum Hall effect]].
| |
| | |
| ======Charge density spread over a wave function======
| |
| | |
| The charge density is not actually concentrated in a delta function. The charge is spread over a wave function. In that case the electron density is<ref>Ezewa, p. 189</ref>
| |
| | |
| : <math>
| |
| {1 \over \pi r_B^2 L_B}
| |
| {1 \over n!}
| |
| \left( {r \over r_B} \right)^{2 \mathit l}
| |
| \exp \left( -{r^2 \over r_B^2} \right)
| |
| .</math>
| |
| | |
| The interaction energy becomes
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| :<math>
| |
| E=
| |
|
| |
| \left( { 2 e^2 \over L_B}\right) \int_0^{\infty} {{k\;dk \;} \over
| |
| k^2 + k_B^2 r_{B}^2 }
| |
| \; M \left ( \mathit l + 1, 1, -{k^2 \over 4} \right) \;M \left ( \mathit l^{\prime} + 1, 1, -{k^2 \over 4} \right) \;\mathcal J_0 \left ( k{r_{12}\over r_{B}} \right)
| |
| </math>
| |
| |}
| |
| | |
| where <math>M</math> is a [[confluent hypergeometric function]] or [[Kummer function]]. In obtaining the interaction energy we have used the integral (see [[Common integrals in quantum field theory#Integration over a magnetic wave function|Common integrals in quantum field theory]])
| |
| | |
| :<math>
| |
| {2 \over n!}
| |
| \int_0^{\infty} { dr }\;r^{2n+1}\exp\left( -r^2\right) J_{0} \left( kr \right)
| |
| =
| |
| M\left( n+1, 1, -{k^2 \over 4}\right)
| |
| . </math>
| |
| | |
| As with delta function charges, the value of <math>r_{12}</math> in which the energy is a local minimum only depends on the total angular momentum, not on the angular momenta of the individual currents. Also, as with the delta function charges, the energy at the minimum increases as the ratio of angular momenta varies from one. Therefore, the series
| |
| | |
| :<math>{\mathit l \over \mathit l^*} ={1\over 3}, {2\over 5}, {3\over 7}, \mbox{etc.,} </math>
| |
| | |
| and
| |
| | |
| :<math>{\mathit l \over \mathit l^*} ={2\over3}, {3\over 5}, {4\over 7}, \mbox{etc.,} </math>
| |
| | |
| appear as well in the case of charges spread by the wave function.
| |
| | |
| The [[Laughlin wavefunction]] is an [[ansatz]] for the quasiparticle wavefunction. If the expectation value of the interaction energy is taken over a [[Laughlin wavefunction]], these series are also preserved.
| |
| | |
| ===Magnetostatics===
| |
| | |
| ====Darwin interaction in a vacuum====
| |
| | |
| A charged moving particle can generate a magnetic field that affects the motion of another charged particle. The static version of this effect is called the [[Darwin Lagrangian|Darwin interaction]]. To calculate this, consider the electrical currents in space generated by a moving charge
| |
| | |
| :<math>
| |
| \vec J_1\left( \vec x \right) = a_1 \vec v_1 \delta^3 \left( \vec x - \vec x_1 \right)
| |
| </math>
| |
| | |
| with a comparable expression for <math> \vec J_2 </math>.
| |
| | |
| The Fourier transform of this current is
| |
| | |
| :<math>
| |
| \vec J_1\left( \vec k \right) = a_1 \vec v_1 \exp\left( i \vec k \cdot \vec x_1 \right)
| |
| .</math>
| |
| | |
| The current can be decomposed into a transverse and a longitudinal part (see [[Helmholtz decomposition]]).
| |
| | |
| :<math>
| |
| \vec J_1\left( \vec k \right) = a_1 \left[ 1 - \hat k \hat k \right ] \cdot \vec v_1 \exp\left( i \vec k \cdot \vec x_1 \right)
| |
| + a_1 \left[ \hat k \hat k \right ] \cdot \vec v_1 \exp\left( i \vec k \cdot \vec x_1 \right)
| |
| .</math>
| |
| | |
| The hat indicates a [[unit vector]]. The last term disappears because
| |
| | |
| :<math>
| |
| \vec k \cdot \vec J = -k_0 J^0 \rightarrow 0
| |
| ,</math>
| |
| | |
| which results from charge conservation. Here <math>k_0 </math> vanishes because we are considering static forces.
| |
| | |
| With the current in this form the energy of interaction can be written
| |
| | |
| :<math> E =
| |
| a_1 a_2\int {d^3k \over (2 \pi )^3 } \; \; D\left ( k \right )\mid_{k_0=0} \;
| |
| \vec v_1 \cdot \left[ 1 - \hat k \hat k \right ] \cdot \vec v_2 \; \exp\left ( i \vec k \cdot \left ( x_1 - x_2 \right ) \right )
| |
| </math>.
| |
| | |
| The propagator equation for the Proca Lagrangian is
| |
| | |
| :<math>
| |
| \eta_{\mu \alpha} \left ( \partial^2 + m^2\right ) D^{\alpha \nu}\left ( x-y \right ) = \delta_{\mu }^{ \nu} \delta^4\left ( x-y \right )
| |
| .</math>
| |
| | |
| The [[spacelike]] solution is
| |
| | |
| :<math>
| |
| D\left ( k \right )\mid_{k_0=0}\; = \;
| |
| -{1 \over \vec k^2 + m^2}
| |
| ,</math>
| |
| | |
| which yields
| |
| | |
| :<math> E =
| |
| - a_1 a_2\int {d^3k \over (2 \pi )^3 } \; \;
| |
| {\vec v_1 \cdot \left[ 1 - \hat k \hat k \right ] \cdot \vec v_2 \over \vec k^2 + m^2 } \; \exp\left ( i \vec k \cdot \left ( x_1 - x_2 \right ) \right )
| |
| </math>
| |
| | |
| which evaluates to (see [[Common integrals in quantum field theory#Transverse potential with mass|Common integrals in quantum field theory]])
| |
| | |
| :<math> E =
| |
| - {1\over 2} {a_1 a_2 \over 4 \pi r } e^{ - m r } \left\{
| |
| {2 \over \left( mr \right)^2 } \left( e^{mr} -1 \right) - {2\over mr} \right \}
| |
| \vec v_1 \cdot \left[ 1 + {\hat r} {\hat r}\right]\cdot \vec v_2
| |
| </math>
| |
| | |
| which reduces to
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math> E =
| |
| - {1\over 2} {a_1 a_2 \over 4 \pi r }
| |
| \vec v_1 \cdot \left[ 1 + {\hat r} {\hat r}\right]\cdot \vec v_2
| |
| </math>
| |
| |}
| |
| | |
| in the limit of small m. The interaction energy is the negative of the interaction Lagrangian. For two like part particles traveling in the same direction, the interaction is attractive, which is the opposite of the Coulomb interaction.
| |
| | |
| ====Darwin interaction in a plasma====
| |
| | |
| In a plasma, the [[dispersion relation]] for an [[electromagnetic wave]] is<ref>Chen, pp. 100-103</ref> (<math>c=1</math>)
| |
| | |
| :<math>
| |
| k_0^2 = \omega_p^2 +\vec k^2
| |
| ,</math>
| |
| | |
| which implies
| |
| | |
| :<math>
| |
| D\left ( k \right )\mid_{k_0=0}\; = \;
| |
| -{1 \over \vec k^2 + \omega_p^2}
| |
| .</math>
| |
| | |
| Here <math>\omega_p</math> is the [[plasma frequency]]. The interaction energy is therefore
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math> E =
| |
| - {1\over 2} {a_1 a_2 \over 4 \pi r }
| |
| \vec v_1 \cdot \left[ 1 + {\hat r} {\hat r}\right]\cdot \vec v_2
| |
| \; e^{ - \omega_p r } \left\{
| |
| {2 \over \left( \omega_p r \right)^2 } \left( e^{\omega_p r} -1 \right) - {2\over \omega_p r} \right \}
| |
| .</math>
| |
| |}
| |
| | |
| ====Magnetic interaction between current loops in a simple plasma or electron gas====
| |
| | |
| =====The interaction energy=====
| |
| | |
| Consider a tube of current rotating in a magnetic field embedded in a simple [[Plasma (physics)|plasma]] or [[electron gas]]. The current, which lies in the plane perpendicular to the magnetic field, is defined as
| |
| | |
| :<math>
| |
| \vec J_1\left( \vec x \right) = a_1 v_1 {1\over 2 \pi r L_B} \; \delta^ 2 \left( r - r_{B1} \right)\;
| |
| \left( {\hat b \times \hat r }\right)
| |
| </math>
| |
| | |
| where
| |
| | |
| :<math>
| |
| r_{B1}
| |
| =
| |
| {\sqrt{4 \pi}m_1v_1\over a_1 B}
| |
| </math>
| |
| | |
| and <math>
| |
| \hat b
| |
| </math> is the unit vector in the direction of the magnetic field. Here <math>L_B</math> indicates the dimension of the material in the direction of the magnetic field. The transverse current, perpendicular to the [[wave vector]], drives the [[transverse wave]].
| |
| | |
| The energy of interaction is
| |
| | |
| :<math>
| |
| E=
| |
| \left( { a_1\, a_2 \over 2 \pi L_B}\right) v_1\, v_2\, \int_0^{\infty} {k\;dk \;} D\left( k \right) \mid_{k_0=k_B=0}
| |
| \mathcal J_1 \left ( kr_{B1} \right) \mathcal J_1 \left ( kr_{B2} \right) \mathcal J_0 \left ( kr_{12} \right)
| |
| </math>
| |
| | |
| where <math>r_{12}</math> is the distance between the centers of the current loops and
| |
| | |
| :<math>
| |
| \mathcal J_n \left ( x \right)
| |
| </math>
| |
| | |
| is a [[Bessel function]] of the first kind. In obtaining the interaction energy we made use of the integrals
| |
| | |
| :<math>
| |
| \int_0^{2 \pi} {d\varphi \over 2 \pi} \exp\left( i p \cos\left( \varphi \right) \right)
| |
| =
| |
| \mathcal J_0 \left( p \right)
| |
| </math>
| |
| | |
| and
| |
| | |
| :<math>
| |
| \int_0^{2 \pi} {d\varphi \over 2 \pi} \cos\left( \varphi \right) \exp\left( i p \cos\left( \varphi \right) \right)
| |
| =
| |
| i\mathcal J_1 \left( p \right)
| |
| . </math>
| |
| | |
| See [[Common integrals in quantum field theory#Angular integration in cylindrical coordinates|Common integrals in quantum field theory]].
| |
| | |
| A current in a plasma confined to the plane perpendicular to the magnetic field generates an [[Electromagnetic electron wave#X wave|extraordinary wave]].<ref>Chen, pp. 110-112</ref> This wave generates [[Hall current]]s that interact and modify the electromagnetic field. The [[dispersion relation]] for extraordinary waves is<ref>Chen, p. 112</ref>
| |
| | |
| :<math>
| |
| -k_0^2 +\vec k^2 + \omega_p^2 { \left( k_0^2 - \omega_p^2\right) \over \left( k_0^2- \omega_H^2 \right) } =0
| |
| ,</math>
| |
| | |
| which gives for the propagator
| |
| | |
| :<math>
| |
| D\left( k \right) \mid_{k_0=k_B=0}\;
| |
| = \;
| |
| -\left( {1\over \vec k^2 + k_X^2}\right)
| |
| </math>
| |
| | |
| where
| |
| | |
| :<math>
| |
| k_X \equiv {\omega_p^2 \over \omega_H}
| |
| </math>
| |
| | |
| in analogy with the Darwin propagator. Here, the upper hybrid frequency is given by
| |
| | |
| :<math>
| |
| \omega_H^2 = \omega_p^2 + \omega_c^2
| |
| ,</math>
| |
| | |
| the [[cyclotron frequency]] is given by ([[Gaussian units]])
| |
| | |
| :<math>
| |
| \omega_c = {e B \over m c}
| |
| ,</math>
| |
| | |
| and the [[plasma frequency]] ([[Gaussian units]])
| |
| | |
| :<math>
| |
| \omega_p^2 = {4\pi n e^2 \over m}
| |
| .</math>
| |
| | |
| Here n is the electron density, e is the magnitude of the electron charge, and m is the electron mass.
| |
| | |
| The interaction energy becomes, for like currents,
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E=
| |
| - \left( { a^2 \over 2 \pi L_B}\right) v^2\, \int_0^{\infty} {k\;dk \over \vec k^2 + k_X^2}
| |
| \mathcal J_1^2 \left ( kr_{B} \right) \mathcal J_0 \left ( kr_{12} \right)
| |
| </math>
| |
| |}
| |
| | |
| =====Limit of small distance between current loops=====
| |
| | |
| In the limit that the distance between current loops is small,
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E=
| |
| - E_0 \;
| |
| I_1 \left( \mu \right)K_1 \left( \mu \right)
| |
| </math>
| |
| |}
| |
| | |
| where
| |
| | |
| <math>
| |
| E_0=
| |
| \left( { a^2 \over 2 \pi L_B}\right) v^2
| |
| </math>
| |
| | |
| and
| |
| | |
| :<math>
| |
| \mu =
| |
| {\omega_p^2 r_B\over \omega_H}
| |
| = k_X \;r_B
| |
| </math>
| |
| | |
| and I and K are modified Bessel functions. we have assumed that the two currents have the same charge and speed.
| |
| | |
| We have made use of the integral (see [[Common integrals in quantum field theory#Integration of the cylindrical propagator with mass|Common integrals in quantum field theory]])
| |
| | |
| :<math>
| |
| \int_o^{\infty} {k\; dk \over k^2 +m^2} \mathcal J_1^2 \left( kr \right)
| |
| =
| |
| I_1 \left( mr \right)K_1 \left( mr \right)
| |
| . </math>
| |
| | |
| For small mr the integral becomes
| |
| | |
| :<math>
| |
| I_1 \left( mr \right)K_1 \left( mr \right)
| |
| \rightarrow
| |
| {1\over 2 }\left[ 1- {1\over 8}\left( mr \right)^2 \right]
| |
| . </math>
| |
| | |
| For large mr the integral becomes
| |
| | |
| :<math>
| |
| I_1 \left( mr \right)K_1 \left( mr \right)
| |
| \rightarrow
| |
| {1\over 2}\;\left( {1\over mr}\right)
| |
| . </math>
| |
| | |
| =====Relation to the quantum Hall effect=====
| |
| | |
| The screening [[wavenumber]] can be written ([[Gaussian units]])
| |
| | |
| :<math>
| |
| \mu =
| |
| {\omega_p^2 r_B\over \omega_H c}
| |
| = \left( {2e^2r_B\over L_B \hbar c }\right) {\nu \over \sqrt{1+{\omega_p^2\over \omega_c^2}}}
| |
| = 2 \alpha \left( { r_B\over L_B }\right) \left({1 \over \sqrt{1+{\omega_p^2\over \omega_c^2}}}\right) \nu
| |
| </math>
| |
| | |
| where <math>\alpha</math> is the [[fine-structure constant]] and the filling factor is
| |
| | |
| :<math>
| |
| \nu =
| |
| {2\pi N \hbar c \over eBA}
| |
| </math>
| |
| | |
| and N is the number of electrons in the material and A is the area of the material perpendicular to the magnetic field. This parameter is important in the [[quantum Hall effect]] and the [[fractional quantum Hall effect]]. The filling factor is the fraction of occupied [[Landau levels|Landau states]] at the ground state energy.
| |
| | |
| For cases of interest in the quantum Hall effect, <math>\mu</math> is small. In that case the interaction energy is
| |
| | |
| ::{|cellpadding="2" style="border:2px solid #ccccff"
| |
| |
| |
| <math>
| |
| E=
| |
| - {E_0\over 2} \left[ 1- {1\over 8}\mu^2\right]
| |
| </math>
| |
| |}
| |
| | |
| where ([[Gaussian units]])
| |
| | |
| :<math>
| |
| E_0=
| |
| {4\pi}{ e^2 \over L_B}{v^2\over c^2}
| |
| = {8\pi}{ e^2 \over L_B}\left( {\hbar \omega_c\over m c^2}\right)
| |
| </math>
| |
| | |
| is the interaction energy for zero filling factor. We have set the classical kinetic energy to the quantum energy
| |
| | |
| :<math>
| |
| {1\over 2} m v^2
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| = \hbar \omega_c
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| .</math>
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| ===Gravitation===
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| The Lagrangian for the gravitational field is [[Spin (physics)|spin]]-2. The disturbance is generated by the [[stress-energy tensor]] <math> T^{\mu \nu} </math>. If the disturbances are at rest, then the only component of the stress-energy tensor that survives is the <math> 00 </math> component. If we use the same trick of giving the [[graviton]] some mass and then taking the mass to zero at the end of the calculation the propagator becomes
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| :<math>
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| D\left ( k \right )\mid_{k_0=0}\; = \; - {4\over 3}
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| {1 \over \vec k^2 + m^2}
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| </math>
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| and
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| ::{|cellpadding="2" style="border:2px solid #ccccff"
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| <math>
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| E =
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| -{4\over 3}{a_1 a_2 \over 4 \pi r } \exp \left ( -m r \right )
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| </math>,
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| |}
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| which is once again attractive rather than repulsive. The coefficients are proportional to the masses of the disturbances. In the limit of small graviton mass, we recover the inverse-square behavior of Newton's Law.<ref>Zee, pp. 32-37</ref>
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| Unlike the electrostatic case, however, taking the small-mass limit of the boson does not yield the correct result. A more rigorous treatment yields a factor of one in the energy rather than 4/3.<ref>Zee, p. 35</ref>
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| ==References==
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| {{Reflist}}<!--added under references heading by script-assisted edit-->
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| [[Category:Quantum field theory]]
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