Nonlinear optics

Nonlinear optics (NLO) is the branch of optics that describes the behavior of light in nonlinear media, that is, media in which the dielectric polarization P responds nonlinearly to the electric field E of the light. This nonlinearity is typically only observed at very high light intensities (values of the electric field comparable to interatomic electric fields, typically 108 V/m) such as those provided by lasers. Above the Schwinger limit, the vacuum itself is expected to become nonlinear. In nonlinear optics, the superposition principle no longer holds.

Nonlinear optics remained unexplored until the discovery in 1961 of Second harmonic generation by Peter Franken et al. at University of Michigan, shortly after the construction of the first laser by Theodore Harold Maiman.[1]

Nonlinear optical processes

Nonlinear optics explains nonlinar response of properties such as frequency, polarization, phase or path of incident light.[1] These nonlinear interactions give rise to a host of optical phenomena:

Frequency mixing processes

Other nonlinear processes

Related processes

In these processes, the medium has a linear response to the light, but the properties of the medium are affected by other causes:

Parametric processes

Nonlinear effects fall into two qualitatively different categories, parametric and non-parametric effects. A parametric non-linearity is an interaction in which the quantum state of the nonlinear material is not changed by the interaction with the optical field. As a consequence of this, the process is 'instantaneous'; Energy and momentum conserving in the optical field, making phase matching important; and polarization dependent.[7] [8]

Theory

Parametric and 'instantaneous' (i.e. material must be lossless and dispersionless through the Kramers-Kronig relations) nonlinear optical phenomena, in which the optical fields are not too large, can be described by a Taylor series expansion of the dielectric Polarization density (dipole moment per unit volume) P(t) at time t in terms of the electrical field E(t):

\mathbf{P}(t) = \varepsilon_0( \chi^{(1)} \mathbf{E}(t) + \chi^{(2)} \mathbf{E}^2(t) + \chi^{(3)} \mathbf{E}^3(t) + \ldots )\ .

Here, the coefficients χ(n) are the n-th order susceptibilities of the medium and the presence of such a term is generally referred to as an n-th order nonlinearity. Note that the polarization density P(t) and electrical field E(t) are considered as scalar for simplicity. In general, χ(n) is an n+1 order tensor representing both the polarization dependent nature of the parametric interaction as well as the symmetries (or lack of) of the nonlinear material.

Wave-equation in a nonlinear material

Central to the study of electromagnetic waves is the wave equation. Starting with Maxwell's equations in an isotropic space containing no free charge, it can be shown that:

\nabla \times \nabla \times \mathbf{E} + \frac{n^2}{c^2}\frac{\partial^2}{\partial t^2}\mathbf{E} = -\frac{1}{\varepsilon_0 c^2}\frac{\partial^2}{\partial t^2}\mathbf{P}^{NL},

where PNL is the nonlinear part of the Polarization density and n is the refractive index which comes from the linear term in P.

Note one can normally use the vector identity

\nabla \times \left( \nabla \times \mathbf{V} \right) = \nabla \left( \nabla \cdot \mathbf{V} \right) - \nabla^2 \mathbf{V}

and Gauss's law (assuming no free charges, \rho_\text{free} = 0),

\nabla\cdot\mathbf{D} = 0,

to obtain the more familiar wave equation

\nabla^2 \mathbf{E} - \frac{n^2}{c^2}\frac{\partial^2}{\partial t^2}\mathbf{E} = 0.

For nonlinear medium Gauss's law does not imply that the identity

\nabla\cdot\mathbf{E} = 0

is true in general, even for an isotropic medium. However even when this term is not identically 0, it is often negligibly small and thus in practice is usually ignored giving us the standard nonlinear wave-equation:

\nabla^2 \mathbf{E} - \frac{n^2}{c^2}\frac{\partial^2}{\partial t^2}\mathbf{E} = \frac{1}{\varepsilon_0 c^2}\frac{\partial^2}{\partial t^2}\mathbf{P}^{NL}.

Nonlinearities as a wave mixing process

The nonlinear wave-equation is an inhomogeneous differential equation. The general solution comes from the study of ordinary differential equations and can be solved by the use of a Green's function. Physically one gets the normal electromagnetic wave solutions to the homogeneous part of the wave equation:

\nabla^2 \mathbf{E} - \frac{n^2}{c^2}\frac{\partial^2}{\partial t^2}\mathbf{E}= 0.

and the inhomogeneous term

\frac{1}{\varepsilon_0 c^2}\frac{\partial^2}{\partial t^2}\mathbf{P}^{NL},

acts as a driver/source of the electromagnetic waves. One of the consequences of this is a nonlinear interaction that will result in energy being mixed or coupled between different frequencies which is often called a 'wave mixing'.

In general an n-th order will lead to n+1-th wave mixing. As an example, if we consider only a second order nonlinearity (three-wave mixing), then the polarization, P, takes the form

\mathbf{P}^{NL}= \varepsilon_0 \chi^{(2)} \mathbf{E}^2(t).

If we assume that E(t) is made up of two components at frequencies ω1 and ω2, we can write E(t) as

\mathbf{E}(t) = E_1\cos(\omega_1t)+E_2\cos(\omega_2t)

and using Euler's formula to convert to exponentials

\mathbf{E}(t) = \frac{1}{2}E_1e^{-i\omega_1t}+\frac{1}{2}E_2e^{-i\omega_2t} + c.c.

where c.c. stands for complex conjugate. Plugging this into the expression for P gives

\begin{align} \mathbf{P}^{NL}= \varepsilon_0 \chi^{(2)} \mathbf{E}^2(t) &= \frac{\varepsilon_0}{4} \chi^{(2)} [ |E_1|^2e^{-i2\omega_1t}+|E_2|^2e^{-i2\omega_2t}\\ &\qquad+2E_1E_2e^{-i(\omega_1+\omega_2)t}\\ &\qquad+2E_1E_2^*e^{-i(\omega_1-\omega_2)t}\\ &\qquad+\left(|E_1|^2+|E_2|^2\right)e^{0} +c.c.], \end{align}

which has frequency components at 2ω1, 2ω2, ω1+ω2, ω1-ω2, and 0. These three-wave mixing processes correspond to the nonlinear effects known as second harmonic generation, sum frequency generation, difference frequency generation and optical rectification respectively.

Note: Parametric generation and amplification is a variation of difference frequency generation, where the lower-frequency of one of the two generating fields is much weaker (parametric amplification) or completely absent (parametric generation). In the latter case, the fundamental quantum-mechanical uncertainty in the electric field initiates the process.

Phase matching

Most transparent materials, like the BK7 glass shown here, have normal dispersion: The index of refraction decreases monotonically as a function of wavelength (or increases as a function of frequency). This makes phase-matching impossible in most frequency-mixing processes. For example, in SHG, there is no simultaneous solution to \omega'=2\omega and k'=2k in these materials. Birefringent materials avoid this problem by having two indices of refraction at once.[9]

The above ignores the position dependence of the electrical fields. In a typical situation, the electrical fields are traveling waves described by

E_j(\mathbf{x},t) = e^{i(\mathbf{k}_j \cdot \mathbf{x} - \omega_j t)} + c.c.,

at position \mathbf{x}, with the wave vector \left \|\mathbf{k}_j\right \| = n(\omega_j)\omega_j/c, where c is the velocity of light in vacuum and n(\omega_j) is the index of refraction of the medium at angular frequency \omega_j. Thus, the second-order polarization at angular frequency \omega_3=\omega_1+\omega_2 is

P^{(2)} (\mathbf{x}, t) \propto E_1^{n_1} E_2^{n_2} e^{i ((\mathbf{k}_1 + \mathbf{k}_2)\cdot\mathbf{x} - \omega_3 t)} + c.c.

At each position \mathbf{x} within the nonlinear medium, the oscillating second-order polarization radiates at angular frequency \omega_3 and a corresponding wave vector \left \|\mathbf{k}_3\right \| = n(\omega_3)\omega_3/c. Constructive interference, and therefore a high intensity \omega_3 field, will occur only if

\vec{\mathbf{k}}_3 = \vec{\mathbf{k}}_1 + \vec{\mathbf{k}}_2.

The above equation is known as the phase matching condition. Typically, three-wave mixing is done in a birefringent crystalline material (I.e., the refractive index depends on the polarization and direction of the light that passes through.), where the polarizations of the fields and the orientation of the crystal are chosen such that the phase-matching condition is fulfilled. This phase matching technique is called angle tuning. Typically a crystal has three axes, one or two of which have a different refractive index than the other one(s). Uniaxial crystals, for example, have a single preferred axis, called the extraordinary (e) axis, while the other two are ordinary axes (o) (see crystal optics). There are several schemes of choosing the polarizations for this crystal type. If the signal and idler have the same polarization, it is called "Type-I phase-matching", and if their polarizations are perpendicular, it is called "Type-II phase-matching". However, other conventions exist that specify further which frequency has what polarization relative to the crystal axis. These types are listed below, with the convention that the signal wavelength is shorter than the idler wavelength.

Phase-matching types (\lambda_p \leq \lambda_s \leq \lambda_i)
Polarizations Scheme
Pump Signal Idler
e o o Type I
e o e Type II (or IIA)
e e o Type III (or IIB)
e e e Type IV
o o o Type V (or Type-0[10] or Zero)
o o e Type VI (or IIB or IIIA)
o e o Type VII (or IIA or IIIB)
o e e Type VIII (or I)

Most common nonlinear crystals are negative uniaxial, which means that the e axis has a smaller refractive index than the o axes. In those crystals, type I and II phasematching are usually the most suitable schemes. In positive uniaxial crystals, types VII and VIII are more suitable. Types II and III are essentially equivalent, except that the names of signal and idler are swapped when the signal has a longer wavelength than the idler. For this reason, they are sometimes called IIA and IIB. The type numbers V–VIII are less common than I and II and variants.

One undesirable effect of angle tuning is that the optical frequencies involved do not propagate collinearly with each other. This is due to the fact that the extraordinary wave propagating through a birefringent crystal possesses a Poynting vector that is not parallel with the propagation vector. This would lead to beam walk-off which limits the nonlinear optical conversion efficiency. Two other methods of phase matching avoids beam walk-off by forcing all frequencies to propagate at a 90 degree angle with respect to the optical axis of the crystal. These methods are called temperature tuning and quasi-phase-matching.

Temperature tuning is where the pump (laser) frequency polarization is orthogonal to the signal and idler frequency polarization. The birefringence in some crystals, in particular Lithium Niobate is highly temperature dependent. The crystal is controlled at a certain temperature to achieve phase matching conditions.

The other method is quasi-phase matching. In this method the frequencies involved are not constantly locked in phase with each other, instead the crystal axis is flipped at a regular interval Λ, typically 15 micrometres in length. Hence, these crystals are called periodically poled. This results in the polarization response of the crystal to be shifted back in phase with the pump beam by reversing the nonlinear susceptibility. This allows net positive energy flow from the pump into the signal and idler frequencies. In this case, the crystal itself provides the additional wavevector k=2π/λ (and hence momentum) to satisfy the phase matching condition. Quasi-phase matching can be expanded to chirped gratings to get more bandwidth and to shape an SHG pulse like it is done in a dazzler. SHG of a pump and Self-phase modulation (emulated by second order processes) of the signal and an optical parametric amplifier can be integrated monolithically.

Higher-order frequency mixing

The above holds for \chi^{(2)} processes. It can be extended for processes where \chi^{(3)} is nonzero, something that is generally true in any medium without any symmetry restrictions; in particular resonantly enhanced sum or difference frequency mixing in gasses is frequently used for extreme or "vacuum" Ultra Violet light generation.[11] In common scenarios, such as mixing in dilute gases, the non-linearity is weak and so the light beams are focused which, unlike the plane wave approximation used above, introduces a pi phase shift on each light beam, complicating the phase matching requirements.[11] Conveniently, difference frequency mixing with \chi^{(3)} cancels this focal phase shift and often has a nearly self-canceling overall phase matching condition, which relatively simplifies broad wavelength tuning compared to sum frequency generation.[11] In \chi^{(3)} all four frequencies are mixing simultaneously, as opposed to sequential mixing via two \chi^{(2)} processes.

The Kerr effect can be described as a \chi^{(3)} as well. At high peak powers the Kerr effect can cause filamentation of light in air, in which the light travels without dispersion or divergence in a self-generated waveguide.[12] At even high intensities the Taylor series, which led the domination of the lower orders, does not converge anymore and instead a time based model is used. When a noble gas atom is hit by an intense laser pulse, which has an electric field strength comparable to the Coulomb field of the atom, the outermost electron may be ionized from the atom. Once freed, the electron can be accelerated by the electric field of the light, first moving away from the ion, then back toward it as the field changes direction. The electron may then recombine with the ion, releasing its energy in the form of a photon. The light is emitted at every peak of the laser light field which is intense enough, producing a series of attosecond light flashes. The photon energies generated by this process can extend past the 800th harmonic order up to a few KeV. This is called high-order harmonic generation. The laser must be linearly polarized, so that the electron returns to the vicinity of the parent ion. High-order harmonic generation has been observed in noble gas jets, cells, and gas-filled capillary waveguides.

Example uses of nonlinear optics

Frequency doubling

One of the most commonly used frequency-mixing processes is frequency doubling or second-harmonic generation. With this technique, the 1064-nm output from Nd:YAG lasers or the 800-nm output from Ti:sapphire lasers can be converted to visible light, with wavelengths of 532 nm (green) or 400 nm (violet), respectively.

Practically, frequency-doubling is carried out by placing a nonlinear medium in a laser beam. While there are many types of nonlinear media, the most common media are crystals. Commonly used crystals are BBO (β-barium borate), KDP (potassium dihydrogen phosphate), KTP (potassium titanyl phosphate), and lithium niobate. These crystals have the necessary properties of being strongly birefringent (necessary to obtain phase matching, see below), having a specific crystal symmetry and of course being transparent for both the impinging laser light and the frequency doubled wavelength, and have high damage thresholds which make them resistant against the high-intensity laser light.

Optical phase conjugation

It is possible, using nonlinear optical processes, to exactly reverse the propagation direction and phase variation of a beam of light. The reversed beam is called a conjugate beam, and thus the technique is known as optical phase conjugation[13][14] (also called time reversal, wavefront reversal and retroreflection).

One can interpret this nonlinear optical interaction as being analogous to a real-time holographic process.[15] In this case, the interacting beams simultaneously interact in a nonlinear optical material to form a dynamic hologram (two of the three input beams), or real-time diffraction pattern, in the material. The third incident beam diffracts off this dynamic hologram, and, in the process, reads out the phase-conjugate wave. In effect, all three incident beams interact (essentially) simultaneously to form several real-time holograms, resulting in a set of diffracted output waves that phase up as the "time-reversed" beam. In the language of nonlinear optics, the interacting beams result in a nonlinear polarization within the material, which coherently radiates to form the phase-conjugate wave.

Comparison of a phase conjugate mirror with a conventional mirror. With the phase conjugate mirror the image is not deformed when passing through an aberrating element twice.[16]

The most common way of producing optical phase conjugation is to use a four-wave mixing technique, though it is also possible to use processes such as stimulated Brillouin scattering. A device producing the phase conjugation effect is known as a phase conjugate mirror (PCM).

For the four-wave mixing technique, we can describe four beams (j = 1,2,3,4) with electric fields:

\Xi_j(\mathbf{x},t) = \frac{1}{2} E_j(\mathbf{x}) e^{i (\omega_j t - \mathbf{k}\cdot\mathbf{x})} + \text{c.c.}

where Ej are the electric field amplitudes. Ξ1 and Ξ2 are known as the two pump waves, with Ξ3 being the signal wave, and Ξ4 being the generated conjugate wave.

If the pump waves and the signal wave are superimposed in a medium with a non-zero χ(3), this produces a nonlinear polarization field:

P_{\mathrm{NL}} = \varepsilon_0 \chi^{(3)} (\Xi_1 + \Xi_2 + \Xi_3)^3\

resulting in generation of waves with frequencies given by ω = ±ω1 ±ω2 ±ω3 in addition to third harmonic generation waves with ω = 3ω1, 3ω2, 3ω3.

As above, the phase-matching condition determines which of these waves is the dominant. By choosing conditions such that ω = ω1 + ω2 - ω3 and k = k1 + k2 - k3, this gives a polarization field:

P_\omega = \frac{1}{2} \chi^{(3)} \varepsilon_0 E_1 E_2 E_3^* e^{i(\omega t - \mathbf{k} \cdot \mathbf{x} ) } + \text{c.c.}.

This is the generating field for the phase conjugate beam, Ξ4. Its direction is given by k4 = k1 + k2 - k3, and so if the two pump beams are counterpropagating (k1 = -k2), then the conjugate and signal beams propagate in opposite directions (k4 = -k3). This results in the retroreflecting property of the effect.

Further, it can be shown for a medium with refractive index n and a beam interaction length l, the electric field amplitude of the conjugate beam is approximated by

E_4 = \frac{i \omega l}{2 n c} \chi^{(3)} E_1 E_2 E_3^*

(where c is the speed of light). If the pump beams E1 and E2 are plane (counterpropagating) waves, then:

E_4(\mathbf{x}) \propto E_3^*(\mathbf{x});

that is, the generated beam amplitude is the complex conjugate of the signal beam amplitude. Since the imaginary part of the amplitude contains the phase of the beam, this results in the reversal of phase property of the effect.

Note that the constant of proportionality between the signal and conjugate beams can be greater than 1. This is effectively a mirror with a reflection coefficient greater than 100%, producing an amplified reflection. The power for this comes from the two pump beams, which are depleted by the process.

The frequency of the conjugate wave can be different from that of the signal wave. If the pump waves are of frequency ω1 = ω2 = ω, and the signal wave higher in frequency such that ω3 = ω + Δω, then the conjugate wave is of frequency ω4 = ω — Δω. This is known as frequency flipping.

Angular and linear momenta in Optical Phase Conjugation

Optical phase conjugation in the near field performs the reversal of classical rays or retroreflection.

Classical picture

In classical Maxwell electrodynamics a phase-conjugating mirror performs reversal of the Poynting vector:

\vec \mathbf{S} (\vec \mathbf{r},t) = \epsilon_0 c^2 \vec \mathbf{E} (\vec \mathbf{r},t) \times \vec \mathbf{B} (\vec \mathbf{r},t); \vec \mathbf{S}_{out} (\vec \mathbf{r},t) = - \vec \mathbf{S}_{in} (\vec \mathbf{r},t)

which is a linear momentum density of electromagnetic field, where (in) means incident field, (out) means reflected field.[17] In the same way a phase conjugated wave has an opposite angular momentum density vector \vec \mathbf{L} (\vec \mathbf{r},t) with respect to incident field:[18]

\vec \mathbf{L} (\vec \mathbf{r},t) = \vec \mathbf{r} \times \vec \mathbf{S} (\vec \mathbf{r},t) ; \vec \mathbf{L}_{out} (\vec \mathbf{r},t) = - \vec \mathbf{L}_{in} (\vec \mathbf{r},t)

The above identities are valid locally , i.e. in each space point \vec \mathbf{r} in a given moment {t} for an ideal phase conjugating mirror .

Quantum picture


In quantum electrodynamics the photon with energy \mathbf{\hbar} \omega also possesses linear momentum \vec \mathbf{P} = \hbar \vec \mathbf{k} and angular momentum, whose projection on propagation axis is {L_z}=\pm \hbar \ell , where \ell is topological charge of photon or winding number, \mathbf{z} is propagation axis. The angular momentum projection on propagation axis has discrete values \pm \hbar \ell .

In quantum electrodynamics the interpretation of phase conjugation is much simpler compared to classical electrodynamics. The photon reflected from phase conjugating mirror (out) has opposite directions of linear and angular momenta with respect to incident photon (in):

\vec \mathbf{P}_{out} = - \hbar \vec \mathbf{k} = - \vec \mathbf{P}_{in} = \hbar \vec \mathbf{k} ; {L_z}_{_{out}} = - \hbar \ell = - {L_z}_{_{in}} = \hbar \ell

Common SHG materials

(Second Harmonic Generation)

Dark-Red Gallium Selenide in its bulk form.

See also

Notes

  1. 1 2 Rigamonti, Luca (April 2010). "Schiff base metal complexes for second order nonlinear optics" (PDF). La Chimica l'Industria (Società Chimica Italiana) (3): 118–122.
  2. ↑ Experimental observation of relativistic nonlinear Thomson scattering : Abstract : Nature
  3. ↑ Phys. Rev. Lett. 76, 3116 (1996) - Observation of Nonlinear Effects in Compton Scattering
  4. ↑ Archived May 21, 2013 at the Wayback Machine
  5. ↑ http://www.nature.com/nphys/journal/v3/n6/full/nphys595.html
  6. ↑ A.P. Kouzov, N.I. Egorova, M. Chrysos, F. Rachet,Non-linear optical channels of the polarizability induction in a pair of interacting molecules, NANOSYSTEMS: PHYSICS, CHEMISTRY, MATHEMATICS, 2012, 3 (2), P 55
  7. ↑ Paschotta, Rüdiger. "Parametric Nonlinearities". Encyclopedia of Laser Physics and Technology
  8. ↑ See Section Parametric versus Nonparametric Processes, Nonlinear Optics by Robert W. Boyd (3rd ed.), pp. 13-15.
  9. ↑ Robert W. Boyd, Nonlinear optics, Third edition, Chapter 2.3.
  10. ↑ Abolghasem, Payam; Junbo Han; Bhavin J. Bijlani; Amr S. Helmy (2010). "Type-0 second order nonlinear interaction in monolithic waveguides of isotropic semiconductors". Optics Express 18 (12): 12681–12689. doi:10.1364/OE.18.012681. PMID 20588396.
  11. 1 2 3 Strauss, CEM; Funk, DJ (1991). "Broadly tunable difference-frequency generation of VUV using two-photon resonances in H2 and Kr". Optics Lett. 16 (15): 1192.
  12. ↑ Xhao, X.M.; Jones, R.J.; Strauss, C.E.M.; Funk, D.J.; Roberts, J.P.; Taylor, A.J. (1997). "Control of femtosecond pulse filament formation in air through variation of the initial chirp of the pulse". IEEE.
  13. ↑ Scientific American, December 1985, "Phase Conjugation," by Vladimir Shkunov and Boris Zel'dovich.
  14. ↑ Scientific American, January 1986, "Applications of Optical Phase Conjugation," by David M. Pepper.
  15. ↑ Scientific American, October 1990, "The Photorefractive Effect," by David M. Pepper, Jack Feinberg, and Nicolai V. Kukhtarev.
  16. ↑ The Fascinating Behavior of Light in Photorefractive Media | Optics & Photonics News
  17. ↑ A.Yu. Okulov, "Angular momentum of photons and phase conjugation", J. Phys. B: At. Mol. Opt. Phys. v. 41, 101001 (2008)
  18. ↑ A.Y. Okulov, "Optical and Sound Helical structures in a Mandelstam - Brillouin mirror". JETP Lett, v.88, n.8, pp. 561-566 (2008)

References

External links

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