Degree of coherence

In quantum optics, correlation functions are used to characterize the statistical and coherence properties of an electromagnetic field. The degree of coherence is the normalized correlation of electric fields. In its simplest form, termed $g^{(1)}$ , it is useful for quantifying the coherence between two electric fields, as measured in a Michelson or other linear optical interferometer. The correlation between pairs of fields, $g^{(2)}$ , typically is used to find the statistical character of intensity fluctuations. First order correlation is actually the amplitude-amplitude correlation and the second order correlation is the intensity-intensity correlation. It is also used to differentiate between states of light that require a quantum mechanical description and those for which classical fields are sufficient. Analogous considerations apply to any Bose field in subatomic physics, in particular to mesons (cf. Bose–Einstein correlations)

Degree of first-order coherence

The normalized first order correlation function is written as:

Figure 1: This is a plot of g⁽¹⁾ as a function of the delay normalized to the coherence length τ/τ_c. The blue curve is for a coherent state (an ideal laser or a single frequency). The red curve is for Lorentzian chaotic light (e.g. collision broadened). The green curve is for Gaussian chaotic light (e.g. Doppler broadened).

g^{(1)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2)= \frac{\left \langle E^*(\mathbf{r}_1,t_1)E(\mathbf{r}_2,t_2) \right \rangle}{\left [ \left \langle\left | E(\mathbf{r}_1,t_1)\right |^2 \right \rangle \left \langle \left |E(\mathbf{r}_2,t_2)\right |^2 \right \rangle \right ]^{1/2}}

Where <> denotes an ensemble (statistical) average. For non-stationary states, such as pulses, the ensemble is made up of many pulses. When one deals with stationary states, where the statistical properties do not change with time, one can replace the ensemble average with a time average. If we restrict ourselves to plane parallel waves then $\mathbf{r}=z$ . In this case, the result for stationary states will not depend on $t_1$ , but on the time delay $\tau=t_1-t_2$ (or $\tau=t_1-t_2-\frac{z_1-z_2}{c}$ if $z_1 \ne z_2$ ).

This allows us to write a simplified form

g^{(1)}( \tau)= \frac{\left \langle E^*(t)E(t+\tau) \right \rangle}{\left \langle\left | E(t)\right |^2 \right \rangle }

where we now average over t.

In optical interferometers such as the Michelson interferometer, Mach-Zehnder interferometer, or Sagnac interferometer, one splits an electric field into two components, introduces a time delay to one of the components, and then recombines them. The intensity of resulting field is measured as a function of the time delay. The visibility of the resulting interference pattern is given by $|g^{(1)}( \tau)|$ . More generally, when combining two space-time points from a field

visibility=

\left | g^{(1)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2) \right |.

The visibility ranges from zero, for incoherent electric fields, to one, for coherent electric fields. Anything in between is described as partially coherent.

Generally, $g^{(1)}(0)=1$ and $g^{(1)}(\tau)=g^{(1)}(-\tau)^*$ .

Examples of g⁽¹⁾

For light of a single frequency (e.g. laser light): $g^{(1)}(\tau)=e^{-i\omega_0\tau}$

For Lorentzian chaotic light (e.g. collision broadened): $g^{(1)}(\tau)=e^{-i\omega_0\tau-(|\tau|/\tau_c)}$

For Gaussian chaotic light (e.g. Doppler broadened): $g^{(1)}(\tau)=e^{-i\omega_0\tau-\frac{\pi}{2}(\tau/\tau_c)^2}$

Here, $\omega_0$ is the central frequency of the light and $\tau_c$ is the coherence time of the light.

Degree of second-order coherence

The normalised second order correlation function is written as:

Figure 2: This is a plot of g⁽²⁾ as a function of the delay normalized to the coherence length τ/τ_c. The blue curve is for a coherent state (an ideal laser or a single frequency). The red curve is for Lorentzian chaotic light (e.g. collision broadened). The green curve is for Gaussian chaotic light (e.g. Doppler broadened). The chaotic light is super-Poissonian and bunched.

g^{(2)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2)= \frac{\left \langle E^*(\mathbf{r}_1,t_1)E^*(\mathbf{r}_2,t_2)E(\mathbf{r}_1,t_1)E(\mathbf{r}_2,t_2) \right \rangle}{\left \langle\left | E(\mathbf{r}_1,t_1)\right |^2 \right \rangle \left \langle \left |E(\mathbf{r}_2,t_2)\right |^2 \right \rangle }

Note that this is not a generalization of the first-order coherence

If the electric fields are considered classical, we can reorder them to express $g^{(2)}$ in terms of intensities. A plane parallel wave in a stationary state will have

g^{(2)}( \tau)= \frac{\left \langle I(t)I(t+\tau) \right \rangle}{\left \langle I(t) \right \rangle^2 }

The above expression is even, $g^{(2)}(\tau)= g^{(2)}(-\tau)$ For classical fields, one can apply Cauchy-Schwarz inequality to the intensities in the above expression (since they are real numbers) to show that $1 \le g^{(2)}(0) \le \infty$ and that $g^{(2)}(\tau) \le g^{(2)}(0)$ . Nevertheless the second-order coherence for an average over fringe of complementary interferometer outputs of a coherent state is only 0.5 (even though $g^{(2)}=1$ for each phase). And $g^{(2)}$ (calculated from averages) can be reduced down to zero with a proper discriminating trigger level applied to the signal (within the range of coherence).

Examples of g⁽²⁾

Chaotic light of all kinds: $g^{(2)}(\tau) = 1 + | g^{(1)}(\tau)|^2$ . Note the Hanbury-Brown and Twiss effect uses this fact to find $| g^{(1)}(\tau)|$ from a measurement of $g^{(2)}(\tau)$ .

Light of a single frequency: $g^{(2)}(\tau) = 1$

Also, please see photon antibunching for another use of $g^{(2)}$ where $g^{(2)}(0) = 0$ for a single photon source because

g^{(2)}(0)= \frac{\left \langle n(n-1) \right \rangle}{\left \langle n \right \rangle^2 }

where $n$ is the photon number observable.^[1]

Degree of nth-order coherence

A generalization of the first-order coherence

g^{(n)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2;\dots;\mathbf{r}_{2n},t_{2n})= \frac{\left \langle E^*(\mathbf{r}_1,t_1)E^*(\mathbf{r}_2,t_2)\cdots E^*(\mathbf{r}_n,t_n)E(\mathbf{r}_{n+1},t_{n+1})E(\mathbf{r}_{n+2},t_{n+2}) \dots E(\mathbf{r}_{2n},t_{2n}) \right \rangle}{\left [ \left \langle\left | E(\mathbf{r}_1,t_1)\right |^2 \right \rangle \left \langle \left |E(\mathbf{r}_2,t_2)\right |^2 \right \rangle\cdots\left \langle \left |E(\mathbf{r}_{2n},t_{2n})\right |^2 \right \rangle \right ]^{1/2}}

A generalization of the second-order coherence

g^{(n)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2;\dots;\mathbf{r}_n,t_n)= \frac{\left \langle E^*(\mathbf{r}_1,t_1)E^*(\mathbf{r}_2,t_2)\cdots E^*(\mathbf{r}_n,t_n)E(\mathbf{r}_1,t_1)E(\mathbf{r}_2,t_2)\cdots E(\mathbf{r}_n,t_n) \right \rangle}{\left \langle\left | E(\mathbf{r}_1,t_1)\right |^2 \right \rangle \left \langle \left |E(\mathbf{r}_2,t_2)\right |^2 \right \rangle\cdots \left \langle \left |E(\mathbf{r}_n,t_n)\right |^2 \right \rangle }

or in intensities

g^{(n)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2;\dots;\mathbf{r}_n,t_n)= \frac{\langle I(\mathbf{r}_1,t_1) I(\mathbf{r}_2,t_2)\cdots I(\mathbf{r}_n,t_n) \rangle}{\langle I(\mathbf{r}_1,t_1) \rangle \langle I(\mathbf{r}_2,t_2) \rangle \cdots \langle I(\mathbf{r}_n,t_n) \rangle }

Examples of g⁽ⁿ⁾

Light of a single frequency:

g^{(n)}( \mathbf{r}_1,t_1;\mathbf{r}_2,t_2;\dots;\mathbf{r}_n,t_n)=1

Using the first definition: Chaotic light of all kinds: $g^{(n)}(\infty)= 0$

Using the second definition: Chaotic light of all kinds: $g^{(n)}(\infty)= 1$ Chaotic light of all kinds: $g^{(n)}(0)= n!$

Generalization to quantum fields

Figure 3: This is a plot of g⁽²⁾ as a function of the delay normalized to the coherence length τ/τ_c. A value of g⁽²⁾ below the dashed black line can only occur in a quantum mechanical model of light. The red curve shows the g⁽²⁾ of the antibunched and sub-Poissonian light emitted from a single atom driven by a laser beam.

The predictions of $g^{(n)}$ for n > 1 change when the classical fields (complex numbers or c-numbers) are replaced with quantum fields (operators or q-numbers). In general, quantum fields do not necessarily commute, with the consequence that their order in the above expressions can not be simply interchanged.

E^* \rightarrow \hat{E}^-

E \rightarrow \hat{E}^+.

With

\hat{E}^-= -i\left (\frac{\hbar\omega}{2\epsilon_0 V} \right )^{1/2}\hat{a}^\dagger e^{-i(kz-wt)}

we get in the case of stationary light:

g^{(2)} = \frac{\left \langle \hat{a}^\dagger(t) \hat{a}^\dagger(t+\tau) \hat{a}(t+\tau) \hat{a}(t) \right \rangle}{\left \langle \hat{a}^\dagger(t) \hat{a}(t) \right \rangle^2}

Photon bunching

Figure 4: This is a plot of g⁽²⁾ as a function of the delay normalized to the coherence length τ/τ_c. This is an example of a g⁽²⁾ that indicates antibunched light but not sub-Poissonian light.

Figure 5: Photon detections as a function of time for a) antibunching (e.g. light emitted from a single atom), b) random (e.g. a coherent state, laser beam), and c) bunching (chaotic light). τ_c is the coherence time (the time scale of photon or intensity fluctuations).

Light is said to be bunched if $g^{(2)}(\tau) < g^{(2)}(0)$ and antibunched if $g^{(2)}(\tau) > g^{(2)}(0)$ .

References

↑ SINGLE PHOTONS FOR QUANTUM INFORMATION PROCESSING - http://www.stanford.edu/group/yamamotogroup/Thesis/DFthesis.pdf

Degree of coherence