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Optical Phase Space

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Title: Optical Phase Space  
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Optical Phase Space

In quantum optics, an optical phase space is a phase space in which all quantum states of an optical system are described. Each point in the optical phase space corresponds to a unique state of an optical system. For any such system, a plot of the quadratures against each other, possibly as functions of time, is called a phase diagram. If the quadratures are functions of time then the optical phase diagram can show the evolution of a quantum optical system with time.

An optical phase diagram can give insight into the properties and behaviors of the system that might otherwise not be obvious. This can allude to qualities of the system that can be of interest to an individual studying an optical system that would be very hard to deduce otherwise. Another use for an optical phase diagram is that it shows the evolution of the state of an optical system. This can be used to determine the state of the optical system at any point in time.

For convenience the reduced Planck constant is set equal to one and is just a rescaling of the results found throughout this article. That is, \hbar = 1 .

Background information

When developing a quantum theory of light it is very common to use an electromagnetic oscillator as a model.[1] An electromagnetic oscillator is an oscillation of the electric field due to an excitation of the electric field. Since the magnetic field is proportional to the rate of change of the electric field, this too oscillates. This gives rise to such phenomena as light and these are the systems being studied when looking at an optical phase space. These systems obey and evolve according to Maxwell's Equations.

Let u(x,t) be a vector function describing a single mode of an electromagnetic oscillator. For simplicitity, it is assumed that this electromagnetic oscillator is contained in a vacuum. One such example is given by

\mathbf{u}(\mathbf{x},t) = \mathbf{u_{0}}e^{i(\mathbf{k} \cdot \mathbf{x} - wt)}

where u0 is the polarization vector, k is the wave vector, w the frequency, and A\cdot B denotes the dot product between the vectors A and B. This is the equation for a plane wave and is a simple example of such an electromagnetic oscillator. The oscillators being examined could either be free waves in space or some normal mode contained in some cavity.

A single mode of the electromagnetic oscillator is isolated from the rest of the system and examined. Such an oscillator can be described by the annihilation operator as the Hamiltonian is strictly a function of the 'annihilation operator' which is in turn responsible for the time evolution of the system. This can be interpreted as the quantized amplitude with which u can be excited.[1] It can then be shown that the electric field strength (i.e. the electromagnetic oscillator used to model the system) is given by:

\widehat{E}_{i}=u_{i}^{*}(\mathbf{x},t)\widehat{a}^{\dagger} + u_{i}(\mathbf{x},t)\widehat{a}[2]

(where xi is a single component of x, position). The Hamiltonian for an electromagnetic oscillator is found by quantizing the electromagnetic field for this oscillator and the formula is given by:

\widehat{H} = w (\widehat{a}^{\dagger}\widehat{a} + 1/2)[2]

(where w is the frequency of the spatial-temporal mode). The annihilation operator is the bosonic annihilation operator and so it obeys the commutation relation given by:

[\widehat{a},\widehat{a}^{\dagger}] = 1

(which is shown in the article Creation and annihilation operators). The eigenstates of the annihilation operator are called coherent states:

\widehat{a}|\alpha\rangle = \alpha|\alpha\rangle

It is important to note that the annihilation operator is not Hermitian, therefore its eigenvalues \alpha can be complex, an important consequence.

Finally, the photon number is given by the operator \widehat{n} = \widehat{a}^{\dagger} \widehat{a} which gives the number of photons in the given spatial-temporal mode, u.

Quadratures

Operators given by

\widehat q = \tfrac 1 {\sqrt 2}(\widehat a^\dagger + \widehat a)

and

\widehat p = \tfrac i {\sqrt 2}(\widehat a^\dagger - \widehat a)

are called the quadratures and they represent the real and imaginary parts of the complex amplitude represented by \widehat a.[1] The commutation relation between the two quadratures can easily be calculated:

\begin{align} \left[ \widehat q, \widehat p \right] &= \tfrac i 2 [\widehat a^\dagger + \widehat a, \widehat a^\dagger - \widehat a] \\ &= \tfrac i 2 ([\widehat a^\dagger, \widehat a^\dagger] - [\widehat a^\dagger, \widehat a] +

   [\widehat a, \widehat a^\dagger] - [\widehat a, \widehat a]) \\

&= \tfrac i 2 (-(-1) + 1) \\ &= i \end{align}

This looks very similar to the commutation relation of the position and momentum operator. Thus, it can be useful to think of and treat the quadratures as the position and momentum of the oscillator although in fact they are the "in-phase and out-of-phase components of the electric field amplitude of the spatial-temporal mode", or u, and have nothing really to do with the position or momentum of the electromagnetic oscillator (as it is hard to define what is meant by position and momentum for an electromagnetic oscillator).[1]

Properties of quadratures

The eigenstates of the quadrature operators \widehat{q} and \widehat{p} are called the quadrature states. They satisfy the relations:

  • \widehat{q}|q\rangle = q |q\rangle and \widehat{p}|p\rangle = p |p\rangle
  • \langle q | q'\rangle = \delta(q-q') and \langle p | p'\rangle = \delta(p-p')
  • \int_{-\infty}^{\infty} |q\rangle \langle q| dq = 1 and \int_{-\infty}^{\infty} |p\rangle \langle p| dp = 1

as these form complete basis sets.

Important result

The following is an important relation that can be derived from the above which justifies our interpretation that the quadratures are the real and imaginary parts of a complex \alpha (i.e. the in-phase and out-of-phase components of the electromagnetic oscillator)

\langle\alpha|\widehat{q}|\alpha\rangle = 2^{-1/2}(\langle\alpha|\widehat{a}^{\dagger}|\alpha\rangle + \langle\alpha|\widehat{a}|\alpha\rangle) = 2^{-1/2}(\alpha^{*}\langle\alpha|\alpha\rangle + \alpha\langle\alpha|\alpha\rangle)

The following is a relationship that can be used to help evaluate the above and is given by:

\langle\alpha'|\alpha\rangle = e^{(-1/2)(|\alpha'|^{2}+|\alpha|^{2}) + \alpha'^{*}\alpha}[1]

This gives us that:

\langle\alpha|\widehat{q}|\alpha\rangle = 2^{-1/2}(\alpha^{*} + \alpha) = q_{\alpha}
\langle\alpha|\widehat{p}|\alpha\rangle = i2^{-1/2}(\alpha^{*} - \alpha) = p_{\alpha} by a similar method as above.
\alpha = 2^{-1/2}(\langle\alpha|\widehat{q}|\alpha\rangle + i\langle\alpha|\widehat{p}|\alpha\rangle) = 2^{-1/2}(q_{\alpha} + ip_{\alpha})

Thus, \alpha is just a composition of the quadratures.

Another very important property of the coherent states becomes very apparent in this formalism. A coherent state is not a point in the optical phase space but rather a distribution on it. This can be seen via

q_{\alpha} = \langle\alpha|\widehat{q}|\alpha\rangle

and

p_{\alpha} = \langle\alpha|\widehat{p}|\alpha\rangle.

These are only the expectation values of \widehat{q} and \widehat{p} for the state |\alpha\rangle.

It can be shown that the quadratures obey Heisenberg's Uncertainty Principle given by:

\Delta q\Delta p \ge 1/2[1] (where \Delta q and \Delta p are the variances of the distributions of q and p, respectively)

This inequality does not necessarily have to be saturated and a common example of such states are squeezed coherent states. The coherent states are Gaussian probability distributions over the phase space localized around \alpha.

Operators on phase space

It is possible to define operators to move the coherent states around the phase space. These can produce new coherent states and allow us to move around phase space.

Phase-shifting operator

The phase-shifting operator rotates the coherent state by an angle \theta in the optical phase space. This operator is given by:

\widehat{U}(\theta) = e^{-i\theta\widehat{n}} [1]

The important relationship

\widehat{U}(\theta)^{\dagger}\widehat{a}\widehat{U}(\theta) = \widehat{a}e^{-i\theta}

is derived as follows:

d/d\theta (\widehat{U}^{\dagger}\widehat{a}\widehat{U}) = i\widehat{n}\widehat{U}^{\dagger}\widehat{a}\widehat{U} - i\widehat{U}^{\dagger}\widehat{a}\widehat{U}\widehat{n} = \widehat{U}^{\dagger}i[\widehat{n},\widehat{a}]\widehat{U}
= \widehat{U}^{\dagger}i(\widehat{a}^{\dagger}\widehat{a}\widehat{a} - \widehat{a}\widehat{a}^{\dagger}\widehat{a})\widehat{U} = \widehat{U}^{\dagger}i[\widehat{a}^{\dagger},\widehat{a}]\widehat{a}\widehat{U} = -i\widehat{U}^{\dagger}\widehat{a}\widehat{U}

and solving this differential equation yields the desired result.

Thus, using the above it becomes clear that

\widehat{U}(\theta)|\alpha\rangle = |\alpha e^{-i\theta}\rangle,

or a rotation by an angle theta on the coherent state in phase space. The following illustrates this more clearly:

\widehat{a}(\widehat{U}|\alpha\rangle) = \widehat{U}\widehat{a}e^{-i\theta}|\alpha\rangle

(which is obtained using the fact that the phase-shifting operator is unitary)

\widehat{a}(\widehat{U}|\alpha\rangle) = \widehat{U} \alpha e^{-i\theta}|\alpha\rangle = \alpha e^{-i\theta}(\widehat{U}|\alpha\rangle)

Thus,

(\alpha e^{-i\theta}, \widehat{U}|\alpha\rangle)

is the eigenpair of

\widehat{a}\widehat{U}|\alpha\rangle.

From this it is possible to see that

(\alpha e^{-i\theta} = 2^{-1/2}[q_{\alpha} cos(\theta) + p_{\alpha} sin(\theta)] + i2^{-1/2}[-q_{\alpha} csin(\theta) + p_{\alpha} cos(\theta)], \widehat{U}|\alpha\rangle = |\alpha e^{-i\theta}\rangle)

which is another way of expressing the eigenpair which more clearly illustrates the effects of the phase-shifting operator on coherent states.

Displacement operator

The displacement operator takes a coherent state and moves it (by some value) to another coherent state somewhere in the phase space. The displacement operator is given by:

\widehat{D}(\alpha) = e^{\alpha\widehat{a}^{\dagger} - \alpha^{*}\widehat{a}}

The relationship

\widehat{D}^{\dagger}\widehat{a}\widehat{D} = \widehat{a} + \alpha.[1]

can be derived quite easily.

To do this, take an infinitesimal displacement \delta\alpha.

The operators \widehat{D} and \widehat{D}^{\dagger} can be expanded in terms of the identity

e^{x} = \sum_{0}^{\infty}x^{i}/i!

and look at the first order terms and ignore all the higher order terms (all higher order terms are very close to zero as \delta\alpha is very small).

Thus:

\widehat{D}^{\dagger}(\delta\alpha)\widehat{a}\widehat{D}(\delta\alpha) = \sum_{i,j}(\delta\alpha^{*}\widehat{a} - \delta\alpha\widehat{a}^{\dagger})^{i}\widehat{a}(\delta\alpha\widehat{a}^{\dagger}-\delta\alpha^{*}\widehat{a})^{j}/i!j!
=\widehat{a} + (\delta\alpha^{*}\widehat{a} - \delta\alpha\widehat{a}^{\dagger})\widehat{a} + \widehat{a}(\delta\alpha\widehat{a}^{\dagger} - \delta\alpha^{*}\widehat{a}) + O(\delta\alpha^{2},(\delta\alpha^{*})^{2}) (but as given above, the higher order terms are very close to zero and therefore neglected)
=\widehat{a} + \widehat{a}(\delta\alpha\widehat{a}^{\dagger} - \delta\alpha^{*}\widehat{a}) - (\delta\alpha\widehat{a}^{\dagger} - \delta\alpha^{*}\widehat{a})\widehat{a}
=\widehat{a} + [\widehat{a},\delta\alpha\widehat{a}^{\dagger} - \delta\alpha^{*}\widehat{a}] = \widehat{a} + \delta\alpha[\widehat{a},\widehat{a}^{\dagger}] - \delta\alpha^{*}[\widehat{a},\widehat{a}] (use the identity from above)
\widehat{D}^{\dagger}(\delta\alpha)\widehat{a}\widehat{D}(\delta\alpha)=\widehat{a} + \delta\alpha

The above identity can be applied repeatedly in the following fashion to derive the following:

(\widehat{D}^{\dagger}(\delta\alpha))^{k}\widehat{a}(\widehat{D}(\delta\alpha))^{k} = \widehat{a} + k\delta\alpha

Thus, the above identity suggests that repeated use of the displacement operator generates translations in phase space.

Important consequence

The following is an important consequence of the displacement vector.

First note that the displacement operator is a unitary operator. Use

\widehat{D}^{\dagger}(\delta\alpha)\widehat{a}\widehat{D}(\delta\alpha)=\widehat{a} + \delta\alpha

to get:

\widehat{a}\widehat{D}(-\alpha)|\alpha\rangle = \widehat{D}(-\alpha)(\widehat{a} - \alpha)|\alpha\rangle
=\widehat{D}(-\alpha)(\widehat{a}|\alpha\rangle - \alpha|\alpha\rangle)
=\widehat{D}(-\alpha)(\alpha|\alpha\rangle - \alpha|\alpha\rangle)

Thus,

\widehat{a}(\widehat{D}(-\alpha)|\alpha\rangle)=0

or it follows that

\widehat{D}(-\alpha)|\alpha\rangle = |0\rangle

which leads to

|\alpha\rangle=\widehat{D}(\alpha)|0\rangle.

This is important as it suggests that all coherent states are just displacements of the ground state, which in optics is also the vacuum state. That is, any coherent state can be generated via the displacement of the ground state of the electromagnetic oscillator from above.

See also

References

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