QUANTUM HARMONIC OSCILLATOR

The 'quantum harmonic oscillator' is the quantum mechanical analogue of the classical harmonic oscillator. It is one of the most important model systems in quantum mechanics because an arbitrary potential can be approximated as a harmonic potential at the vicinity of a stable equilibrium point. Furthermore, it is one of the few quantum mechanical systems for which a simple exact solution is known.

Contents

One-dimensional harmonic oscillator

Ladder operator method

Natural length and energy scales

Example: diatomic molecules

''N''-dimensional harmonic oscillator

Example: 3D isotropic harmonic oscillator

Coupled harmonic oscillators

See also

References

External links

One-dimensional harmonic oscillator

===Hamiltonian and energy eigenstates===


In the one-dimensional harmonic oscillator problem, a particle of mass ''m'' is subject to a potential ''V''(''x'') = (1/2)''m''ω² ''x''². The Hamiltonian of the particle is:
:
where ''x'' is the position operator, and ''p'' is the momentum operator $left(p\; =\; -i\; hbar\; \{d\; over\; dx\}$
ight). The first term represents the kinetic energy of the particle, and the second term represents the potential energy in which it resides. In order to find the energy levels and the corresponding energy eigenstates, we must solve the time-independent Schrödinger equation,
:$H\; left|\; psi$
ight
angle = E left| psi
ight
angle .
We can solve the differential equation in the coordinate basis, using a power series method. It turns out that there is a family of solutions,
:$leftlangle\; x\; |\; psi\_n$
ight
angle = sqrt{rac{1}{2^n,n!}} cdot left(rac{momega}{pi hbar}
ight)^{1/4} cdot exp
left(- rac{momega x^2}{2 hbar}
ight) cdot H_nleft(sqrt{rac{momega}{hbar}} x
ight)
:$n\; =\; 0,\; 1,\; 2,\; ldots$
The first six solutions (''n'' = 0 to 5) are shown on the right. The functions $H\_n$ are the Hermite polynomials:
:
They should not be confused with the Hamiltonian, which is also denoted by ''H''. The corresponding energy levels are
:$E\_n\; =\; hbar\; omega\; left(n\; +\; \{1over\; 2\}$
ight).
This energy spectrum is noteworthy for three reasons. Firstly, the energies are "quantized", and may only take the discrete values of $hbaromega$ times 1/2, 3/2, 5/2, and so forth. This is a feature of many quantum mechanical systems. In the following section on ladder operators, we will engage in a more detailed examination of this phenomenon. Secondly, the lowest achievable energy is not zero, but $hbaromega/2$, which is called the "ground state energy" or zero-point energy. In the ground state, according to quantum mechanics, an oscillator performs null oscillations and its average kinetic energy is positive. It is not obvious that this is significant, because normally the zero of energy is not a physically meaningful quantity, only differences in energies. Nevertheless, the ground state energy has many implications, particularly in quantum gravity. The final reason is that the energy levels are equally spaced, unlike the Bohr model or the particle in a box.
Note that the ground state probability density is concentrated at the origin. This means the particle spends most of its time at the bottom of the potential well, as we would expect for a state with little energy. As the energy increases, the probability density becomes concentrated at the "classical turning points", where the state's energy coincides with the potential energy. This is consistent with the classical harmonic oscillator, in which the particle spends most of its time (and is therefore most likely to be found) at the turning points, where it is the slowest. The correspondence principle is thus satisfied.

Ladder operator method

The power series solution, though straightforward, is rather tedious. The "ladder operator" method, due to Paul Dirac, allows us to extract the energy eigenvalues without directly solving the differential equation. Furthermore, it is readily generalizable to more complicated problems, notably in quantum field theory. Following this approach, we define the operators ''a'' and its adjoint ''a''^†
:
a &=& sqrt{momega over 2hbar} left(x + {i over m omega} p
ight) \
a^{dagger} &=& sqrt{m omega over 2hbar} left( x - {i over m omega} p
ight)
end{matrix}
The operator ''a'' is not Hermitian since it and its adjoint ''a''^† are not equal.
The operator ''a'' and ''a''^† have properties as below:
:
a left| phi _n
ight
angle &=& sqrt{n} left| phi _{n-1}
ight
angle \
a^{dagger} left| phi _n
ight
angle &=& sqrt{n+1} left| phi _{n+1}
ight
angle
end{matrix}
In deriving the form of ''a''^†, we have used the fact that the operators x and p, which represent observables, ''are'' Hermitian. These observable operators can be expressed as a linear combination of the ladder operators as
:
x &=& sqrt{hbar over 2momega} left( a^{dagger} + a
ight) \
p &=& i sqrt{{hbar}momega over 2} left( a^{dagger} - a
ight)
end{matrix}
The ''x'' and ''p'' operators obey the following identity, known as the canonical commutation relation:
:$left[x\; ,\; p$
ight] = ihbar .
The square brackets in this equation are a commonly-used notational device, known as the commutator, defined as
:$left[A\; ,\; B$
ight] stackrel{mathrm{def}}{=} AB - BA.
Using the above, we can prove the identities
:$H\; =\; hbar\; omega\; left(a^\{dagger\}a\; +\; 1/2$
ight)
:$left[a\; ,\; a^\{dagger\}$
ight] = 1.
Now, let $left|psi\_E$
ight
angle denote an energy eigenstate with energy ''E''. The inner product of any ket with itself must be non-negative, so
:$left(a\; left|psi\_E$
ight
angle, a left|psi_E
ight
angle
ight) = leftlanglepsi_E
ight| a^dagger a left| psi_E
ight
angle ge 0.
Expressing ''a''^†''a'' in terms of the Hamiltonian:
:$leftlanglepsi\_E$
ight| {H over hbar omega} - {1 over 2} left|psi_E
ight
angle = left({E over hbar omega} - {1 over 2}
ight) ge 0,
so that $E\; ge\; hbar\; omega\; /\; 2$. Note that when ($a\; left|\; psi\_E$
ight
angle) is the zero ket (i.e. a ket with length zero), the inequality is saturated, so that $E\; =\; hbar\; omega\; /\; 2$. It is straightforward to check that there exists a state satisfying this condition; it is the ground (''n'' = 0) state given in the preceding section.
Using the above identities, we can now show that the commutation relations of ''a'' and ''a''^† with ''H'' are:
:
left[H , a
ight] &=& - hbar omega a \
left[H , a ^dagger
ight] &=& hbar omega a^dagger
end{matrix}.
Thus, provided ($a\; left|\; psi\_E$
ight
angle) is not the zero ket,
:
H (a left| psi_E
ight
angle)
&=& (left[H,a
ight] + a H) left|psi_E
ight
angle \
&=& (- hbaromega a + a E) left|psi_E
ight
angle \
&=& (E - hbaromega) (aleft|psi_E
ight
angle)
end{matrix}.
Similarly, we can show that
:$H\; (a^dagger\; left|\; psi\_E$
ight
angle) = (E + hbaromega) (a^dagger left| psi_E
ight
angle).
In other words, ''a'' acts on an eigenstate of energy ''E'' to produce, up to a multiplicative constant, another eigenstate of energy $E\; -\; hbar\; omega$, and ''a''^† acts on an eigenstate of energy ''E'' to produce an eigenstate of energy $E\; +\; hbar\; omega$. For this reason, ''a'' is called a "lowering operator", and ''a''^† a "raising operator". The two operators together are called "ladder operators". In quantum field theory, ''a'' and ''a''^† are alternatively called "annihilation" and "creation" operators because they destroy and create particles, which correspond to our quanta of energy.
Given any energy eigenstate, we can act on it with the lowering operator, ''a'', to produce another eigenstate with $hbar\; omega$-less energy. By repeated application of the lowering operator, it seems that we can produce energy eigenstates down to ''E'' = −∞. However, this would contradict our earlier requirement that $E\; ge\; hbar\; omega\; /\; 2$. Therefore, there must be a ground-state energy eigenstate, which we label $left|\; 0$
ight
angle (not to be confused with the zero ket), such that
:$a\; left|\; 0$
ight
angle = 0 hbox{(zero ket)}.
In this case, subsequent applications of the lowering operator will just produce zero kets, instead of additional energy eigenstates. Furthermore, we have shown above that
:$H\; left|0$
ight
angle = (hbaromega/2) left|0
ight
angle
Finally, by acting on $left|\; 0$
ight
angle with the raising operator and multiplying by suitable normalization factors, we can produce an infinite set of energy eigenstates $left\{left|\; 0$
ight
angle, left| 1
ight
angle, left| 2
ight
angle, ... , left| n
ight
angle, ...
ight}, such that
:$H\; left|n$
ight
angle = hbaromega (n + 1/2) left|n
ight
angle
which matches the energy spectrum which we gave in the preceding section.

Natural length and energy scales

The quantum harmonic oscillator possesses natural scales for length and energy, which can be used to simplify the problem. These can be found by nondimensionalization. The result is that if we measure energy in units of $hbar\; omega$ and distance in units of $left(hbar\; /\; left(m\; omega$
ight)
ight)^{1/2}, then the Schrödinger equation becomes:
:$H\; =\; -\; \{1over2\}\; \{d^2\; over\; du^2\; \}\; +\; \{1\; over\; 2\}\; u^2$,
and the energy eigenfunctions and eigenvalues become
:$leftlangle\; x\; |\; psi\_n$
ight
angle = {1 over sqrt{2^n n!}} pi^{-1/4} hbox{exp} (-u^2 / 2) H_n(u)
:$E\_n\; =\; n\; +\; \{1over\; 2\}$.
To avoid confusion, we will not adopt these natural units in this article. However, they frequently come in handy when performing calculations.

Example: diatomic molecules

Main articles: diatomic molecule

In diatomic molecules, the natural frequency can be found by: [1]
:
where
:$omega\; =\; 2\; pi\; f$   is the angular frequency,
:''k'' is the 'bond force constant', and
:$m\_r$ is the reduced mass.

''N''-dimensional harmonic oscillator

The one-dimensional harmonic oscillator is readily generalizable to ''N'' dimensions, where ''N'' = 1, 2, 3, ... . In one dimension, the position of the particle was specified by a single coordinate, ''x''. In ''N'' dimensions, this is replaced by ''N'' position coordinates, which we label ''x''₁, ..., ''x''_''N''. Corresponding to each position coordinate is a momentum; we label these ''p''₁, ..., ''p''_''N''. The canonical commutation relations between these operators are
:
left[x_i , p_j
ight] &=& ihbardelta_{i,j} \
left[x_i , x_j
ight] &=& 0 \
left[p_i , p_j
ight] &=& 0
end{matrix}.
The Hamiltonian for this system is
:$H\; =\; sum\_\{i=1\}^N\; left(\; \{p\_i^2\; over\; 2m\}\; +\; \{1over\; 2\}\; m\; omega^2\; x\_i^2$
ight).
As the form of this Hamiltonian makes clear, the ''N''-dimensional harmonic oscillator is exactly analogous to ''N'' independent one-dimensional harmonic oscillators with the same mass and spring constant. In this case, the quantities ''x''₁, ..., ''x''_''N'' would refer to the positions of each of the ''N'' particles. This is a happy property of the ''r''² potential, which allows the potential energy to be separated into terms depending on one coordinate each.
This observation makes the solution straightforward. For a particular set of quantum numbers {''n''} the energy eigenfunctions for the ''N''-dimensional oscillator are expressed in terms of the 1-dimensional eigenfunctions as:
:$$
langle mathbf{x}|psi_{{n}}
angle
=prod_{i=1}^Nlangle x_i|psi_{n_i}
angle

In the ladder operator method, we define ''N'' sets of ladder operators,
:
a_i &=& sqrt{momega over 2hbar} left(x_i + {i over m omega} p_i
ight) \
a^{dagger}_i &=& sqrt{m omega over 2hbar} left( x_i - {i over m omega} p_i
ight)
end{matrix}.
By a procedure analogous to the one-dimensional case, we can then show that each of the ''a''_''i'' and ''a''^†_''i'' operators lower and raise the energy by ℏω respectively. The Hamiltonian is
:$$
H = hbar omega , sum_{i=1}^N left(a_i^dagger ,a_i + rac{1}{2}
ight).

This Hamiltonian is invariant under the dynamic symmetry group ''U(N)'' (the unitary group in ''N'' dimensions), defined by
:$$
U, a_i^dagger ,U^dagger = sum_{j=1}^N a_j^dagger,U_{ji}quadhbox{for all}quad
U in U(N),

where $U\_\{ji\}$ is an element in the defining matrix representation of ''U(N)''.
The energy levels of the system are
:$E\; =\; hbar\; omega\; left[(n\_1\; +\; cdots\; +\; n\_N)\; +\; \{Nover\; 2\}$
ight].
:$$
n_i = 0, 1, 2, dots quad (hbox{the number of bosons in mode } i).

As in the one-dimensional case, the energy is quantized. The ground state energy is ''N'' times the one-dimensional energy, as we would expect using the analogy to ''N'' independent one-dimensional oscillators. There is one further difference: in the one-dimensional case, each energy level corresponds to a unique quantum state. In ''N''-dimensions, except for the ground state, the energy levels are ''degenerate'', meaning there are several states with the same energy.
The degeneracy can be calculated relatively easily, as an example, consider the 3-dimensional case: Define ''n'' = ''n''₁ + ''n''₂ + ''n''₃. All states with the same ''n'' will have the same energy. For a given ''n'', we choose a particular ''n''₁. Then ''n''₂ + ''n''₃ = ''n'' − ''n''₁. There are ''n'' − ''n''₁ + 1 possible groups {''n''₂, ''n''₃}. ''n''₂ can take on the values 0 to ''n'' − ''n''₁, and for each ''n''₂ the value of ''n''₃ is fixed. The degree of degeneracy therefore is:
:$$
g_n = sum_{n_1=0}^n n - n_1 + 1 = rac{(n+1)(n+2)}{2}

Formula for general ''N'' and ''n'' [''g''_n being the dimension of the symmetric irreducible ''n''^th power representation of the unitary group ''U(N)'']:
:$$
g_n = inom{N+n-1}{n}

The special case ''N = 3'', given above, follows directly from this general equation.

Example: 3D isotropic harmonic oscillator

The Schrödinger equation of a spherically-symmetric three-dimensional harmonic oscillator can be solved explicitly by separation of variables, see this article for the present case. This procedure is analogous to the separation performed in the hydrogen-like atom problem, but with the spherically symmetric potential
:$V(r)\; =\; \{1over\; 2\}\; mu\; omega^2\; r^2,$
where $mu$ is the mass of the problem. Because ''m'' will be used below for the magnetic quantum number, mass is indicated by $mu$, instead of ''m'', as earlier in this article.
The solution reads
:$psi\_\{klm\}(r,\; heta,phi)\; =\; N\_\{kl\}\; r^\{l\}e^\{-$
u r^2}{L_k}^{(l+{1over 2})}(2
u r^2) Y_{lm}( heta,phi)
where
:$N\_\{kl\},$ is a normalization constant.
:$$
u equiv {mu omega over 2 hbar}
:$\{L\_k\}^\{(l+\{1over\; 2\})\}(2$
u r^2) are generalized Laguerre polynomials. The order ''k'' of the polynomial is a non-negative integer.
:$Y\_\{lm\}(\; heta,phi),$ is a spherical harmonic function.
:$hbar$ is the reduced Planck constant: .
The energy eigenvalue is
:$E=hbar\; omega\; (2k+l+\{3over\; 2\})$
The energy is usually described by the single quantum number
:$nequiv\; 2k+l,$
Because ''k'' is a non-negative integer, for every even ''n'' we have $l=0,2...,n-2,n$ and for every odd ''n'' we have $l=1,3...,n-2,n$. The magnetic quantum number ''m'' is an integer satisfying $-l\; le\; m\; le\; l$, so for every ''n'' and ''l'' there are ''2l+1'' different quantum states, labeled by ''m''. Thus, the degeneracy at level ''n'' is
:$sum\_\{l=ldots,n-2,n\}\; (2l+1)\; =\; \{(n+1)(n+2)over\; 2\}$
where the sum starts from 0 or 1, according to whether ''n'' is even or odd.
This result is in accordance with the dimension formula above.

Coupled harmonic oscillators

In this problem, we consider ''N'' equal masses which are connected to their neighbors by springs, in the limit of large ''N''. The masses form a linear chain in one dimension, or a regular lattice in two or three dimensions.
As in the previous section, we denote the positions of the masses by ''x''₁, ''x''₂, ..., as measured from their equilibrium positions (i.e. ''x''_''k'' = 0 if particle ''k'' is at its equilibrium position.) In two or more dimensions, the ''x''s are vector quantities. The Hamiltonian of the total system is
:$H\; =\; sum\_\{i=1\}^N\; \{p\_i^2\; over\; 2m\}\; +\; \{1over\; 2\}\; m\; omega^2\; sum\_\{\{ij\}\; (nn)\}\; (x\_i\; -\; x\_j)^2$
The potential energy is summed over "nearest-neighbor" pairs, so there is one term for each spring.
Remarkably, there exists a coordinate transformation to turn this problem into a set of independent harmonic oscillators, each of which corresponds to a particular collective distortion of the lattice. These distortions display some particle-like properties, and are called phonons. Phonons occur in the ionic lattices of many solids, and are extremely important for understanding many of the phenomena studied in solid state physics.

See also

★ Gas in a harmonic trap

★ Creation and annihilation operators

★ Coherent state

★ Morse potential

References

★ Introduction to Quantum Mechanics (2nd ed.), Griffiths, David J., , , Prentice Hall, 2004, ISBN 0-13-805326-X

★ Introductory Quantum Mechanics, Liboff, Richard L., , , Addison-Wesley, 2002, ISBN 0-8053-8714-5

External links

★ Quantum Harmonic Oscillator

★ Calculation using a noncommutative free monoid: (mathematical version) / (abbreviated version)