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In physics, a **phonon** is a collective excitation in a periodic, elastic arrangement of atoms or molecules in condensed matter, specifically in solids and some liquids. Often designated a quasiparticle,^{[1]} it represents an excited state in the quantum mechanical quantization of the modes of vibrations of elastic structures of interacting particles.

Phonons play a major role in many of the physical properties of condensed matter, such as thermal conductivity and electrical conductivity. The study of phonons is an important part of condensed matter physics.

The concept of phonons was introduced in 1932 by Soviet physicist Igor Tamm. The name *phonon* comes from the Greek word φωνή (*phonē*), which translates to *sound* or *voice* because long-wavelength phonons give rise to sound. The name is analogous to the word *photon*.

A phonon is the quantum mechanical description of an elementary vibrational motion in which a lattice of atoms or molecules uniformly oscillates at a single frequency.^{[2]} In classical mechanics this designates a normal mode of vibration. Normal modes are important because any arbitrary lattice vibration can be considered to be a superposition of these *elementary* vibration modes (cf. Fourier analysis). While normal modes are wave-like phenomena in classical mechanics, phonons have particle-like properties too, in a way related to the wave–particle duality of quantum mechanics.

The equations in this section do not use axioms of quantum mechanics but instead use relations for which there exists a direct correspondence in classical mechanics.

For example: a rigid regular, crystalline (not amorphous), lattice is composed of *N* particles. These particles may be atoms or molecules. *N* is a large number, say of the order of 10^{23}, or on the order of Avogadro's number for a typical sample of a solid. Since the lattice is rigid, the atoms must be exerting forces on one another to keep each atom near its equilibrium position. These forces may be Van der Waals forces, covalent bonds, electrostatic attractions, and others, all of which are ultimately due to the electric force. Magnetic and gravitational forces are generally negligible. The forces between each pair of atoms may be characterized by a potential energy function *V* that depends on the distance of separation of the atoms. The potential energy of the entire lattice is the sum of all pairwise potential energies multiplied by a factor of 1/2 to compensate for double counting:^{[3]}

where *r _{i}* is the position of the

It is difficult to solve this many-body problem explicitly in either classical or quantum mechanics. In order to simplify the task, two important approximations are usually imposed. First, the sum is only performed over neighboring atoms. Although the electric forces in real solids extend to infinity, this approximation is still valid because the fields produced by distant atoms are effectively screened. Secondly, the potentials *V* are treated as harmonic potentials. This is permissible as long as the atoms remain close to their equilibrium positions. Formally, this is accomplished by Taylor expanding *V* about its equilibrium value to quadratic order, giving *V* proportional to the displacement *x*^{2} and the elastic force simply proportional to *x*. The error in ignoring higher order terms remains small if *x* remains close to the equilibrium position.

The resulting lattice may be visualized as a system of balls connected by springs. The following figure shows a cubic lattice, which is a good model for many types of crystalline solid. Other lattices include a linear chain, which is a very simple lattice which we will shortly use for modeling phonons. (For other common lattices, see crystal structure.)

The potential energy of the lattice may now be written as

Here, *ω* is the natural frequency of the harmonic potentials, which are assumed to be the same since the lattice is regular. *R _{i}* is the position coordinate of the

Due to the connections between atoms, the displacement of one or more atoms from their equilibrium positions gives rise to a set of vibration waves propagating through the lattice. One such wave is shown in the figure to the right. The amplitude of the wave is given by the displacements of the atoms from their equilibrium positions. The wavelength *λ* is marked.

There is a minimum possible wavelength, given by twice the equilibrium separation *a* between atoms. Any wavelength shorter than this can be mapped onto a wavelength longer than 2*a*, due to the periodicity of the lattice. This can be thought as one consequence of Nyquist–Shannon sampling theorem, the lattice points are viewed as the "sampling points" of a continuous wave.

Not every possible lattice vibration has a well-defined wavelength and frequency. However, the normal modes do possess well-defined wavelengths and frequencies.

In order to simplify the analysis needed for a 3-dimensional lattice of atoms, it is convenient to model a 1-dimensional lattice or linear chain. This model is complex enough to display the salient features of phonons.

The forces between the atoms are assumed to be linear and nearest-neighbour, and they are represented by an elastic spring. Each atom is assumed to be a point particle and the nucleus and electrons move in step (adiabatic approximation):

*n*− 1*n**n*+ 1 ←*a*→

···o++++++o++++++o++++++o++++++o++++++o++++++o++++++o++++++o++++++o···

- →→ → →→→
*u*_{n − 1}*u*_{n}*u*_{n + 1}

where n labels the nth atom out of a total of N, a is the distance between atoms when the chain is in equilibrium, and *u _{n}* the displacement of the nth atom from its equilibrium position.

If *C* is the elastic constant of the spring and m the mass of the atom, then the equation of motion of the nth atom is

This is a set of coupled equations. Since the solutions are expected to be oscillatory, new coordinates are defined by a discrete Fourier transform, in order to decouple them.^{[4]}

Put

Here, *na* corresponds and devolves to the continuous variable x of scalar field theory. The *Q _{k}* are known as the normal coordinates, continuum field modes

These are the equations for harmonic oscillators which have the solution

Each normal coordinate *Q _{k}* represents an independent vibrational mode of the lattice with wavenumber k which is known as a normal mode.

The second equation, for *ω _{k}*, is known as the dispersion relation between the angular frequency and the wavenumber. In the continuum limit, a→0, N→∞, with

A one-dimensional quantum mechanical harmonic chain consists of *N* identical atoms. This is the simplest quantum mechanical model of a lattice that allows phonons to arise from it. The formalism for this model is readily generalizable to two and three dimensions.

In some contrast to the previous section, the positions of the masses are not denoted by *u _{i}*, but, instead, by

where *m* is the mass of each atom (assuming it is equal for all), and *x _{i}* and

A set of *N* "normal coordinates" *Q _{k}* may be introduced, defined as the discrete Fourier transforms of the

The quantity *k _{n}* turns out to be the wavenumber of the phonon, i.e. 2π divided by the wavelength.

This choice retains the desired commutation relations in either real space or wavevector space

From the general result

The potential energy term is

where

The Hamiltonian may be written in wavevector space as

The couplings between the position variables have been transformed away; if the *Q* and *Π* were Hermitian (which they are not), the transformed Hamiltonian would describe *N* uncoupled harmonic oscillators.

The form of the quantization depends on the choice of boundary conditions; for simplicity, *periodic* boundary conditions are imposed, defining the (*N* + 1)th atom as equivalent to the first atom. Physically, this corresponds to joining the chain at its ends. The resulting quantization is

The upper bound to *n* comes from the minimum wavelength, which is twice the lattice spacing *a*, as discussed above.

The harmonic oscillator eigenvalues or energy levels for the mode *ω _{k}* are:

The levels are evenly spaced at:

where 1/2*ħω* is the zero-point energy of a quantum harmonic oscillator.

An **exact** amount of energy *ħω* must be supplied to the harmonic oscillator lattice to push it to the next energy level. In comparison to the photon case when the electromagnetic field is quantized, the quantum of vibrational energy is called a phonon.

All quantum systems show wavelike and particlelike properties simultaneously. The particle-like properties of the phonon are best understood using the methods of second quantization and operator techniques described later.^{[6]}

This may be generalized to a three-dimensional lattice. The wavenumber *k* is replaced by a three-dimensional wavevector **k**. Furthermore, each **k** is now associated with three normal coordinates.

The new indices *s* = 1, 2, 3 label the polarization of the phonons. In the one-dimensional model, the atoms were restricted to moving along the line, so the phonons corresponded to longitudinal waves. In three dimensions, vibration is not restricted to the direction of propagation, and can also occur in the perpendicular planes, like transverse waves. This gives rise to the additional normal coordinates, which, as the form of the Hamiltonian indicates, we may view as independent species of phonons.

For a one-dimensional alternating array of two types of ion or atom of mass *m*_{1}, *m*_{2} repeated periodically at a distance *a*, connected by springs of spring constant *K*, two modes of vibration result:^{[8]}

where *k* is the wavevector of the vibration related to its wavelength by
.

The connection between frequency and wavevector, *ω* = *ω*(*k*), is known as a dispersion relation. The plus sign results in the so-called *optical* mode, and the minus sign to the *acoustic* mode. In the optical mode two adjacent different atoms move against each other, while in the acoustic mode they move together.

The speed of propagation of an acoustic phonon, which is also the speed of sound in the lattice, is given by the slope of the acoustic dispersion relation, ∂*ω _{k}*/∂

For a crystal that has at least two atoms in its primitive cell, the dispersion relations exhibit two types of phonons, namely, optical and acoustic modes corresponding to the upper blue and lower red curve in the diagram, respectively. The vertical axis is the energy or frequency of phonon, while the horizontal axis is the wavevector. The boundaries at −π/*a* and π/*a* are those of the first Brillouin zone.^{[8]} A crystal with *N* ≥ 2 different atoms in the primitive cell exhibits three acoustic modes: one longitudinal acoustic mode and two transverse acoustic modes. The number of optical modes is 3*N* – 3. The lower figure shows the dispersion relations for several phonon modes in GaAs as a function of wavevector **k** in the principal directions of its Brillouin zone.^{[7]}

Many phonon dispersion curves have been measured by inelastic neutron scattering.

The physics of sound in fluids differs from the physics of sound in solids, although both are density waves: sound waves in fluids only have longitudinal components, whereas sound waves in solids have longitudinal and transverse components. This is because fluids cannot support shear stresses (but see viscoelastic fluids, which only apply to high frequencies).

In fact, the above-derived Hamiltonian looks like the classical Hamiltonian function, but if it is interpreted as an operator, then it describes a quantum field theory of non-interacting bosons.

The energy spectrum of this Hamiltonian is easily obtained by the method of ladder operators, similar to the quantum harmonic oscillator problem. We introduce a set of ladder operators defined by:^{[citation needed]}

By direct insertion on the Hamiltonian, it is readily verified that^{[citation needed]}

As with the quantum harmonic oscillator, one can show that *b _{k}*

Two important properties of phonons may be deduced. Firstly, phonons are bosons, since any number of identical excitations can be created by repeated application of the creation operator *b _{k}*

It is not *a priori* obvious that these excitations generated by the *b* operators are literally waves of lattice displacement, but one may convince oneself of this by calculating the *position–position correlation function*.^{[citation needed]} Let |*k*⟩ denote a state with a single quantum of mode *k* excited, i.e.

One can show that, for any two atoms *j* and *l*,

which has the form of a lattice wave with frequency *ω _{k}* and wavenumber

In three dimensions the Hamiltonian has the form

^{[citation needed]}

Solids with more than one atom in the smallest unit cell exhibit two types of phonons: acoustic phonons and optical phonons.

**Acoustic phonons** are coherent movements of atoms of the lattice out of their equilibrium positions. If the displacement is in the direction of propagation, then in some areas the atoms will be closer, in others farther apart, as in a sound wave in air (hence the name acoustic). Displacement perpendicular to the propagation direction is comparable to waves on a string. If the wavelength of acoustic phonons goes to infinity, this corresponds to a simple displacement of the whole crystal, and this costs zero deformation energy. Acoustic phonons exhibit a linear relationship between frequency and phonon wavevector for long wavelengths. The frequencies of acoustic phonons tend to zero with longer wavelength. Longitudinal and transverse acoustic phonons are often abbreviated as LA and TA phonons, respectively.

**Optical phonons** are out-of-phase movements of the atoms in the lattice, one atom moving to the left, and its neighbour to the right. This occurs if the lattice basis consists of two or more atoms. They are called *optical* because in ionic crystals, like sodium chloride, they are excited by infrared radiation. The electric field of the light will move every positive sodium ion in the direction of the field, and every negative chloride ion in the other direction, sending the crystal vibrating.

Optical phonons have a non-zero frequency at the Brillouin zone center and show no dispersion near that long wavelength limit. This is because they correspond to a mode of vibration where positive and negative ions at adjacent lattice sites swing against each other, creating a time-varying electrical dipole moment. Optical phonons that interact in this way with light are called *infrared active*. Optical phonons that are *Raman active* can also interact indirectly with light, through Raman scattering. Optical phonons are often abbreviated as LO and TO phonons, for the longitudinal and transverse modes respectively; the splitting between LO and TO frequencies is often described accurately by the Lyddane–Sachs–Teller relation.

When measuring optical phonon energy by experiment, optical phonon frequencies are sometimes given in spectroscopic wavenumber notation, where the symbol *ω* represents ordinary frequency (not angular frequency), and is expressed in units of cm^{−1}. The value is obtained by dividing the frequency by the speed of light in vacuum. In other words, the frequency in cm^{−1} units corresponds to the inverse of the wavelength of a photon in vacuum, that has the same frequency as the measured phonon.^{[9]} The cm^{−1} is a unit of energy used frequently in the dispersion relations of both acoustic and optical phonons, see units of energy for more details and uses.

By analogy to photons and matter waves, phonons have been treated with wavevector *k* as though it has a momentum *ħk*,^{[10]} however, this is not strictly correct, because *ħk* is not actually a physical momentum; it is called the *crystal momentum* or *pseudomomentum*. This is because *k* is only determined up to addition of constant vectors (the reciprocal lattice vectors and integer multiples thereof). For example, in the one-dimensional model, the normal coordinates *Q* and *Π* are defined so that

where

for any integer *n*. A phonon with wavenumber *k* is thus equivalent to an infinite family of phonons with wavenumbers *k* ± 2π/*a*, *k* ± 4π/*a*, and so forth. Physically, the reciprocal lattice vectors act as additional chunks of momentum which the lattice can impart to the phonon. Bloch electrons obey a similar set of restrictions.

It is usually convenient to consider phonon wavevectors *k* which have the smallest magnitude |*k*| in their "family". The set of all such wavevectors defines the *first Brillouin zone*. Additional Brillouin zones may be defined as copies of the first zone, shifted by some reciprocal lattice vector.

The thermodynamic properties of a solid are directly related to its phonon structure. The entire set of all possible phonons that are described by the phonon dispersion relations combine in what is known as the phonon density of states which determines the heat capacity of a crystal. By the nature of this distribution, the heat capacity is dominated by the high-frequency part of the distribution, while thermal conductivity is primarily the result of the low-frequency region.^{[citation needed]}

At absolute zero temperature, a crystal lattice lies in its ground state, and contains no phonons. A lattice at a nonzero temperature has an energy that is not constant, but fluctuates randomly about some mean value. These energy fluctuations are caused by random lattice vibrations, which can be viewed as a gas of phonons. Because these phonons are generated by the temperature of the lattice, they are sometimes designated thermal phonons.^{[citation needed]}

Thermal phonons can be created and destroyed by random energy fluctuations. In the language of statistical mechanics this means that the chemical potential for adding a phonon is zero. This behavior is an extension of the harmonic potential into the anharmonic regime. The behavior of thermal phonons is similar to the photon gas produced by an electromagnetic cavity, wherein photons may be emitted or absorbed by the cavity walls. This similarity is not coincidental, for it turns out that the electromagnetic field behaves like a set of harmonic oscillators, giving rise to Black-body radiation. Both gases obey the Bose–Einstein statistics: in thermal equilibrium and within the harmonic regime, the probability of finding phonons or photons in a given state with a given angular frequency is:^{[citation needed]}

where *ω*_{k,s} is the frequency of the phonons (or photons) in the state, *k*_{B} is Boltzmann's constant, and *T* is the temperature.

The idea of quantum tunneling applied to phonons produces the idea of *phonon tunneling*, where across nanometer-wide gaps, heat can transfer between materials from phonon that "tunnel" between the two materials.^{[11]} The type of heat transfer works between distances too large for conduction to occur but too small for radiation to occur.

The phonon Hamiltonian is given by

In terms of the operators, these are given by

Here, in expressing the Hamiltonian in operator formalism, we have not taken into account the 1/2*ħω _{q}* term, since if we take an infinite lattice or, for that matter a continuum, the 1/2

The ground state also called the "vacuum state" is the state composed of no phonons. Hence, the energy of the ground state is 0. When, a system is in state |*n*_{1}*n*_{2}*n*_{3}…⟩, we say there are *n _{α}* phonons of type

and,

i.e. *a _{α}*

The number operator commutes with a string of products of the creation and annihilation operators if, the number of *a* are equal to number of *a*^{†}.

Phonons are bosons, since |*α*,*β*⟩ = |*β*,*α*⟩ i.e. they are symmetric under exchange.^{[12]}

As well as photons, phonons can interact via parametric down conversion^{[13]} and form squeezed coherent states.^{[14]}

Even though phonons are often used as a quasiparticle, some popular research has shown that phonons and rotons may indeed have some kind of mass and be affected by gravity as standard particles are.^{[15]} In particular, phonons are predicted to have a kind of negative mass and negative gravity.^{[16]} This can be explained by how phonons are known to travel faster in denser materials. Because the part of a material pointing towards a gravitational source is closer to the object, it becomes denser on that end. From this, it is predicted that phonons would deflect away as it detects the difference in densities, exhibiting the qualities of a negative gravitational field.^{[17]} Although the effect would be too small to measure, it is possible that future equipment could lead to successful results.

Phonons have also been predicted to play a key role in superconductivity in materials and the prediction of superconductive compounds.^{[18]}

In 2019, researchers were able to isolate individual phonons without destroying them for the first time.^{[19]}

**^**Schwabl, Franz (2008).*Advanced Quantum Mechanics*(4th ed.). Springer. p. 253. ISBN 978-3-540-85062-5.**^**Simon, Steven H. (2013).*The Oxford solid state basics*(1st ed.). Oxford: Oxford University Press. p. 82. ISBN 978-0-19-968077-1.**^**Krauth, Werner (April 2006).*Statistical mechanics: algorithms and computations*. International publishing locations: Oxford University Press. pp. 231–232. ISBN 978-0-19-851536-4.**^**Mattuck, R.*A guide to Feynman Diagrams in the many-body problem*.**^**Fetter, Alexander; Walecka, John (2003-12-16).*Theoretical Mechanics of Particles and Continua*. Dover Books on Physics. ISBN 978-0486432618.**^**Mahan, G. D. (1981).*Many-Particle Physics*. New York: Springer. ISBN 978-0-306-46338-9.- ^
^{a}^{b}Yu, Peter Y.; Cardona, Manuel (2010). "Fig. 3.2: Phonon dispersion curves in GaAs along high-symmetry axes".*Fundamentals of Semiconductors*. Physics and Materials Properties (4th ed.). Springer. p. 111. ISBN 978-3-642-00709-5. - ^
^{a}^{b}Misra, Prasanta Kumar (2010). "§2.1.3 Normal modes of a one-dimensional chain with a basis".*Physics of Condensed Matter*. Academic Press. p. 44. ISBN 978-0-12-384954-0. **^**Mahan, Gerald (2010).*Condensed Matter in a Nutshell*. Princeton: Princeton University Press. ISBN 978-0-691-14016-2.**^**Kittel, Charles (2004).*Introduction to Solid State Physics, 8th Edition*. Wiley. p. 100. ISBN 978-0-471-41526-8.**^**"Tunneling across a tiny gap".*News.mit.edu*. Retrieved 13 August 2019.**^**Feynman, Richard P. (1982).*Statistical Mechanics, A Set of Lectures*. Reading, MA: Benjamin-Cummings. p. 159. ISBN 978-0-8053-2508-9.**^**Marquet, C.; Schmidt-Kaler, F.; James, D. F. V. (2003). "Phonon–phonon interactions due to non-linear effects in a linear ion trap" (PDF).*Applied Physics B*.**76**(3): 199–208. arXiv:quant-ph/0211079. Bibcode:2003ApPhB..76..199M. doi:10.1007/s00340-003-1097-7.**^**Reiter, D. E.; Sauer, S.; Huneke, J.; Papenkort, T.; Kuhn, T.; Vagov, A.; Axt, V. M. (2009). "Generation of squeezed phonon states by optical excitation of a quantum dot" (PDF).*Journal of Physics: Conference Series*. Institute of Physics.**193**: 012121. doi:10.1088/1742-6596/193/1/012121.**^**Alberto Nicolis and Riccardo Penco. (2017). Mutual Interactions of Phonons, Rotons, and Gravity, Arxiv.org, Retrieved November 27, 2018**^**Angelo Esposito, Rafael Krichevsky, and Alberto Nicolis. (2018). The mass of sound Retrieved November 11, 2018**^**"Researchers suggest phonons may have mass and perhaps negative gravity".*Phys.org*. Retrieved 13 August 2019.**^**Enamul Haque and M. Anwar Hossain. (2018). prediction of phonon-mediated superconductivity in XBC (X= Mg, Ca, Sr, Ba) Arviv.org, Retrieved November 27, 2018**^**"Detecting the softest sounds in the Universe".*Nature*. July 1, 2019. Retrieved August 13, 2019.

Wikimedia Commons has media related to .Lattice vibrations |

- Explained: Phonons, MIT News, 2010.
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