Gaussian beam

File:Gaussian beam w40mm lambda30mm.png

Instantaneous absolute value of the real part of electric field amplitude of a TEM₀₀ Gaussian beam, focal region. Showing $|{ℛ}{ℯ}(E(t_1))|$ thus with two peaks for each positive wavefront.

File:Laser gaussian profile.svg

Top: transverse intensity profile of a Gaussian beam that is propagating out of the page. Blue curve: electric (or magnetic) field amplitude vs. radial position from the beam axis. The black curve is the corresponding intensity.

File:Green laser pointer TEM00 profile.JPG

A 5 mW green laser pointer beam, showing the TEM₀₀ profile

In optics, a Gaussian beam is an idealized beam of electromagnetic radiation whose amplitude envelope in the transverse plane is given by a Gaussian function; this also implies a Gaussian intensity (irradiance) profile. This fundamental (or TEM₀₀) transverse Gaussian mode describes the intended output of many lasers, as such a beam diverges less and can be focused better than any other. When a Gaussian beam is refocused by an ideal lens, a new Gaussian beam is produced. The electric and magnetic field amplitude profiles along a circular Gaussian beam of a given wavelength and polarization are determined by two parameters: the waist w₀, which is a measure of the width of the beam at its narrowest point, and the position Template:Mvar relative to the waist.

Since the Gaussian function is infinite in extent, perfect Gaussian beams do not exist in nature, and the edges of any such beam would be cut off by any finite lens or mirror. However, the Gaussian is a useful approximation to a real-world beam for cases where lenses or mirrors in the beam are significantly larger than the spot size w(z) of the beam.

Fundamentally, the Gaussian is a solution of the paraxial Helmholtz equation, the wave equation for an electromagnetic field. Although there exist other solutions, the Gaussian families of solutions are useful for problems involving compact beams.

Mathematical form

The equations below assume a beam with a circular cross-section at all values of Template:Mvar; this can be seen by noting that a single transverse dimension, Template:Mvar, appears. Beams with elliptical cross-sections, or with waists at different positions in Template:Mvar for the two transverse dimensions (astigmatic beams) can also be described as Gaussian beams, but with distinct values of w₀ and of the z = 0 location for the two transverse dimensions Template:Mvar and Template:Mvar.

File:Gaussian-beam intensity surfaceplot.png

Gaussian beam intensity profile with w₀ = 2λ.

The Gaussian beam is a transverse electromagnetic (TEM) mode. The mathematical expression for the electric field amplitude is a solution to the paraxial Helmholtz equation. Assuming polarization in the Template:Mvar direction and propagation in the +z direction, the electric field in phasor (complex) notation is given by:

$$\mathbf{𝐄}(r,z)=E_0\widehat{\mathbf{𝐱}}\frac{w_0}{w(z)}\exp \left(\frac{-r^2}{w(z{)}^2}\right)\exp (-i(kz+k\frac{r^2}{2R(z)}-\psi (z)))$$

where

• Template:Mvar is the radial distance from the center axis of the beam,
• Template:Mvar is the axial distance from the beam's focus (or "waist"),
• Template:Mvar is the imaginary unit,
• k = 2πn/λ is the wave number (in radians per meter) for a free-space wavelength Template:Mvar, and Template:Mvar is the index of refraction of the medium in which the beam propagates,
• E₀ = E(0, 0), the electric field amplitude at the origin (r = 0, z = 0),
• w(z) is the radius at which the field amplitudes fall to 1/e of their axial values (i.e., where the intensity values fall to 1/e² of their axial values), at the plane Template:Mvar along the beam,
• w₀ = w(0) is the waist radius,
• R(z) is the radius of curvature of the beam's wavefronts at Template:Mvar, and
• ψ(z) = arctan(z/z_R) is the Gouy phase at Template:Mvar, an extra phase term beyond that attributable to the phase velocity of light.

The physical electric field is obtained from the phasor field amplitude given above by taking the real part of the amplitude times a time factor: $${\mathbf{𝐄}}_{\text{phys}}(r,z,t)=\mathrm{Re}(\mathbf{𝐄}(r,z)\cdot e^{i\omega t}),$$ where $\omega$ is the angular frequency of the light and Template:Mvar is time. The time factor involves an arbitrary sign convention, as discussed at Template:Section link.

Since this solution relies on the paraxial approximation, it is not accurate for very strongly diverging beams. The above form is valid in most practical cases, where w₀ ≫ λ/n.

The corresponding intensity (or irradiance) distribution is given by

$$I(r,z)=\frac{|E(r,z){|}^2}{2\eta }=I_0{\left(\frac{w_0}{w(z)}\right)}^2\exp \left(\frac{-2r^2}{w(z{)}^2}\right),$$

where the constant Template:Mvar is the wave impedance of the medium in which the beam is propagating. For free space, η = η₀ ≈ 377 Ω. I₀ = Template:Mabs²/2η is the intensity at the center of the beam at its waist.

If P₀ is the total power of the beam, $$I_0=\frac{2P_0}{\pi w_0^2}.$$

Evolving beam width

File:Gaussian Beam FWHM.gif

The Gaussian function has a 1/e² diameter (2w as used in the text) about 1.7 times the FWHM.

At a position Template:Mvar along the beam (measured from the focus), the spot size parameter Template:Mvar is given by a hyperbolic relation: $$w(z)=w_0\sqrt{1+{\left(\frac{z}{z_{\mathrm{R}}}\right)}^2},$$ where $$z_{\mathrm{R}}=\frac{\pi w_0^{2}n}{\lambda }$$ is called the Rayleigh range as further discussed below, and $n$ is the refractive index of the medium.

The radius of the beam w(z), at any position Template:Mvar along the beam, is related to the full width at half maximum (FWHM) of the intensity distribution at that position according to: $$w(z)=\frac{\text{FWHM}(z)}{\sqrt{2\ln 2}}.$$

Wavefront curvature

The wavefronts have zero curvature (radius = ∞) at the waist. Wavefront curvature increases in magnitude away from the waist, reaching an extremum at the Rayleigh distance, z = ±z_R (maximum for z = +z_R, minimum for z = -z_R). Beyond the Rayleigh distance, Template:Mabs > z_R, the curvature again decreases in magnitude, approaching zero as z → ±∞. The curvature is often expressed in terms of its reciprocal, Template:Mvar, the radius of curvature; for a fundamental Gaussian beam the curvature at position Template:Mvar is given by:

$$\frac{1}{R(z)}=\frac{z}{z^2+z_{\mathrm{R}}^2},$$

so the radius of curvature R(z) is $$R(z)=z\left[1+{\left(\frac{z_{\mathrm{R}}}{z}\right)}^2\right].$$ Being the reciprocal of the curvature, the radius of curvature reverses sign and is infinite at the beam waist where the curvature goes through zero.

Elliptical and astigmatic beams

Many laser beams have an elliptical cross-section. Also common are beams with waist positions which are different for the two transverse dimensions, called astigmatic beams. These beams can be dealt with using the above two evolution equations, but with distinct values of each parameter for Template:Mvar and Template:Mvar and distinct definitions of the z = 0 point. The Gouy phase is a single value calculated correctly by summing the contribution from each dimension, with a Gouy phase within the range ±π/4 contributed by each dimension.

An elliptical beam will invert its ellipticity ratio as it propagates from the far field to the waist. The dimension which was the larger far from the waist, will be the smaller near the waist.

Gaussian as a decomposition into modes

Arbitrary solutions of the paraxial Helmholtz equation can be decomposed as the sum of Hermite–Gaussian modes (whose amplitude profiles are separable in Template:Mvar and Template:Mvar using Cartesian coordinates), Laguerre–Gaussian modes (whose amplitude profiles are separable in Template:Mvar and Template:Mvar using cylindrical coordinates) or similarly as combinations of Ince–Gaussian modes (whose amplitude profiles are separable in Template:Mvar and Template:Mvar using elliptical coordinates). At any point along the beam Template:Mvar these modes include the same Gaussian factor as the fundamental Gaussian mode multiplying the additional geometrical factors for the specified mode. However different modes propagate with a different Gouy phase which is why the net transverse profile due to a superposition of modes evolves in Template:Mvar, whereas the propagation of any single Hermite–Gaussian (or Laguerre–Gaussian) mode retains the same form along a beam.

Although there are other modal decompositions, Gaussians are useful for problems involving compact beams, that is, where the optical power is rather closely confined along an axis. Even when a laser is not operating in the fundamental Gaussian mode, its power will generally be found among the lowest-order modes using these decompositions, as the spatial extent of higher order modes will tend to exceed the bounds of a laser's resonator (cavity). "Gaussian beam" normally implies radiation confined to the fundamental (TEM₀₀) Gaussian mode.

Beam parameters

The geometric dependence of the fields of a Gaussian beam are governed by the light's wavelength Template:Mvar (in the dielectric medium, if not free space) and the following beam parameters, all of which are connected as detailed in the following sections.

Beam waist

File:GaussianBeamWaist.svg

Gaussian beam width w(z) as a function of the distance Template:Mvar along the beam, which forms a hyperbola. w₀: beam waist; Template:Mvar: depth of focus; z_R: Rayleigh range; Template:Mvar: total angular spread

The shape of a Gaussian beam of a given wavelength Template:Mvar is governed solely by one parameter, the beam waist w₀. This is a measure of the beam size at the point of its focus (z = 0 in the above equations) where the beam width w(z) (as defined above) is the smallest (and likewise where the intensity on-axis (r = 0) is the largest). From this parameter the other parameters describing the beam geometry are determined. This includes the Rayleigh range z_R and asymptotic beam divergence Template:Mvar, as detailed below.

Rayleigh range and confocal parameter

The Rayleigh distance or Rayleigh range z_R is determined given a Gaussian beam's waist size:

$$z_{\mathrm{R}}=\frac{\pi w_0^{2}n}{\lambda }.$$

Here Template:Mvar is the wavelength of the light, Template:Mvar is the index of refraction. At a distance from the waist equal to the Rayleigh range z_R, the width Template:Mvar of the beam is

1. REDIRECT Template:Radic

Template:Rcat shell larger than it is at the focus where w = w₀, the beam waist. That also implies that the on-axis (r = 0) intensity there is one half of the peak intensity (at z = 0). That point along the beam also happens to be where the wavefront curvature (1/R) is greatest.

The distance between the two points z = ±z_R is called the confocal parameter or depth of focus of the beam.

Beam divergence

Although the tails of a Gaussian function never actually reach zero, for the purposes of the following discussion the "edge" of a beam is considered to be the radius where r = w(z). That is where the intensity has dropped to 1/e² of its on-axis value. Now, for z ≫ z_R the parameter w(z) increases linearly with Template:Mvar. This means that far from the waist, the beam "edge" (in the above sense) is cone-shaped. The angle between that cone (whose r = w(z)) and the beam axis (r = 0) defines the divergence of the beam: $$\theta =\underset{z\to \mathrm{\infty }}{\lim }\arctan \left(\frac{w(z)}{z}\right).$$

In the paraxial case, as we have been considering, Template:Mvar (in radians) is then approximately $$\theta =\frac{\lambda }{\pi n{w}_0}$$

where Template:Mvar is the refractive index of the medium the beam propagates through, and Template:Mvar is the free-space wavelength. The total angular spread of the diverging beam, or apex angle of the above-described cone, is then given by $$\mathrm{\Theta }=2\theta .$$

That cone then contains 86% of the Gaussian beam's total power.

Because the divergence is inversely proportional to the spot size, for a given wavelength Template:Mvar, a Gaussian beam that is focused to a small spot diverges rapidly as it propagates away from the focus. Conversely, to minimize the divergence of a laser beam in the far field (and increase its peak intensity at large distances) it must have a large cross-section (w₀) at the waist (and thus a large diameter where it is launched, since w(z) is never less than w₀). This relationship between beam width and divergence is a fundamental characteristic of diffraction, and of the Fourier transform which describes Fraunhofer diffraction. A beam with any specified amplitude profile also obeys this inverse relationship, but the fundamental Gaussian mode is a special case where the product of beam size at focus and far-field divergence is smaller than for any other case.

Since the Gaussian beam model uses the paraxial approximation, it fails when wavefronts are tilted by more than about 30° from the axis of the beam. From the above expression for divergence, this means the Gaussian beam model is only accurate for beams with waists larger than about 2λ/π.

Laser beam quality is quantified by the beam parameter product (BPP). For a Gaussian beam, the BPP is the product of the beam's divergence and waist size w₀. The BPP of a real beam is obtained by measuring the beam's minimum diameter and far-field divergence, and taking their product. The ratio of the BPP of the real beam to that of an ideal Gaussian beam at the same wavelength is known as M² ("M squared"). The M² for a Gaussian beam is one. All real laser beams have M² values greater than one, although very high quality beams can have values very close to one.

The numerical aperture of a Gaussian beam is defined to be NA = n sin θ, where Template:Mvar is the index of refraction of the medium through which the beam propagates. This means that the Rayleigh range is related to the numerical aperture by $$z_{\mathrm{R}}=\frac{n{w}_0}{\mathrm{N}\mathrm{A}}.$$

Gouy phase

The Gouy phase is a phase shift gradually acquired by a beam around the focal region. At position Template:Mvar the Gouy phase of a fundamental Gaussian beam is given by $$\psi (z)=\arctan \left(\frac{z}{z_{\mathrm{R}}}\right).$$

File:Bildschirmfoto 2020-07-05 um 12.50.52.png

Gouy phase.

The Gouy phase results in an increase in the apparent wavelength near the waist (z ≈ 0). Thus the phase velocity in that region formally exceeds the speed of light. That paradoxical behavior must be understood as a near-field phenomenon where the departure from the phase velocity of light (as would apply exactly to a plane wave) is very small except in the case of a beam with large numerical aperture, in which case the wavefronts' curvature (see previous section) changes substantially over the distance of a single wavelength. In all cases the wave equation is satisfied at every position.

The sign of the Gouy phase depends on the sign convention chosen for the electric field phasor. With e^iωt dependence, the Gouy phase changes from -π/2 to +π/2, while with e^-iωt dependence it changes from +π/2 to -π/2 along the axis.

For a fundamental Gaussian beam, the Gouy phase results in a net phase discrepancy with respect to the speed of light amounting to Template:Mvar radians (thus a phase reversal) as one moves from the far field on one side of the waist to the far field on the other side. This phase variation is not observable in most experiments. It is, however, of theoretical importance and takes on a greater range for higher-order Gaussian modes.

Power through an aperture

If a Gaussian beam is centered on a circular aperture of radius Template:Mvar at distance Template:Mvar from the beam waist, the power Template:Mvar that passes through the aperture is $$P(r,z)=P_0[1-e^{-2r^2/w^2(z)}],$$

For a circle of radius r = w(z), the fraction of power transmitted through the circle is $$\frac{P(w(z),z)}{P_0}=1-e^{-2}\approx 0.865.$$

Similarly, about 90% of the beam's power will flow through a circle of radius r = 1.07 × w(z), 95% through a circle of radius r = 1.224 × w(z), and 99% through a circle of radius r = 1.52 × w(z).

Complex beam parameter

Template:Main article The spot size and curvature of a Gaussian beam as a function of Template:Mvar along the beam can also be encoded in the complex beam parameter q(z) given by: $$q(z)=z+i{z}_{\mathrm{R}}.$$

The reciprocal of q(z) contains the wavefront curvature and relative on-axis intensity in its real and imaginary parts, respectively:

$$\frac{1}{q(z)}=\frac{1}{R(z)}-i\frac{\lambda }{n\pi w^2(z)}.$$

The complex beam parameter simplifies the mathematical analysis of Gaussian beam propagation, and especially in the analysis of optical resonator cavities using ray transfer matrices.

Then using this form, the earlier equation for the electric (or magnetic) field is greatly simplified. If we call Template:Mvar the relative field strength of an elliptical Gaussian beam (with the elliptical axes in the Template:Mvar and Template:Mvar directions) then it can be separated in Template:Mvar and Template:Mvar according to: $$u(x,y,z)=u_x(x,z)u_y(y,z),$$

where $$\begin{array}{rl}{u}_x(x,z)& =\frac{1}{\sqrt{q_x(z)}}\exp (-ik\frac{x^2}{2q_x(z)}),\\ u_y(y,z)& =\frac{1}{\sqrt{q_y(z)}}\exp (-ik\frac{y^2}{2q_y(z)}),\end{array}$$

where q_x(z) and q_y(z) are the complex beam parameters in the Template:Mvar and Template:Mvar directions.

For the common case of a circular beam profile, q_x(z) = q_y(z) = q(z) and x² + y² = r², which yields $$u(r,z)=\frac{1}{q(z)}\exp (-ik\frac{r^2}{2q(z)}).$$

Beam optics

File:Gaussian Beam and Lens Diagram.svg

A diagram of a gaussian beam passing through a lens.

When a gaussian beam propagates through a thin lens, the outgoing beam is also a (different) gaussian beam, provided that the beam travels along the cylindrical symmetry axis of the lens, and that the lens is larger than the width of the beam. The focal length of the lens $f$, the beam waist radius $w_0$, and beam waist position $z_0$ of the incoming beam can be used to determine the beam waist radius ${w_0}^{\prime }$ and position ${z_0}^{\prime }$ of the outgoing beam.

Lens equation

As derived by Saleh and Teich, the relationship between the ingoing and outgoing beams can be found by considering the phase that is added to each point $(x,y)$ of the gaussian beam as it travels through the lens. An alternative approach due to Self is to consider the effect of a thin lens on the gaussian beam wavefronts.

The exact solution to the above problem is expressed simply in terms of the magnification $M$

$\begin{array}{rl}{w_0}^{\prime }& =M{w}_0\\ ({z_0}^{\prime }-f)& =M^2(z_0-f).\end{array}$

The magnification, which depends on $w_0$ and $z_0$, is given by

$M=\frac{M_r}{\sqrt{1+r^2}}$

where

$r=\frac{z_R}{z_0-f},M_r=\left|\frac{f}{z_0-f}\right|.$

An equivalent expression for the beam position ${z_0}^{\prime }$ is

$\frac{1}{z_0+\frac{z_R^2}{(z_0-f)}}+\frac{1}{{z_0}^{\prime }}=\frac{1}{f}.$

This last expression makes clear that the ray optics thin lens equation is recovered in the limit that $\left|\left(\frac{z_R}{z_0}\right)\left(\frac{z_R}{z_0-f}\right)\right|\ll 1$. It can also be noted that if $|z_0+\frac{z_R^2}{z_0-f}|\gg f$ then the incoming beam is "well collimated" so that ${z_0}^{\prime }\approx f$.

Beam focusing

In some applications it is desirable to use a converging lens to focus a laser beam to a very small spot. Mathematically, this implies minimization of the magnification $M$. If the beam size is constrained by the size of available optics, this is typically best achieved by sending the largest possible collimated beam through a small focal length lens, i.e. by maximizing $z_R$ and minimizing $f$. In this situation, it is justifiable to make the approximation $z_R^2/(z_0-f{)}^2\gg 1$, implying that $M\approx f/z_R$ and yielding the result ${w_0}^{\prime }\approx f{w}_0/z_R$. This result is often presented in the form

$\begin{array}{rl}2{w_0}^{\prime }& \approx \frac{4}{\pi }\lambda F_{\mathrm{\#}}\\ {z_0}^{\prime }& \approx f\end{array}$

where

$F_{\mathrm{\#}}=\frac{f}{2w_0},$

which is found after assuming that the medium has index of refraction $n\approx 1$ and substituting $z_R=\pi w_0^2/\lambda$. The factors of 2 are introduced because of a common preference to represent beam size by the beam waist diameters $2{w_0}^{\prime }$ and $2w_0$, rather than the waist radii ${w_0}^{\prime }$ and $w_0$.

Wave equation

As a special case of electromagnetic radiation, Gaussian beams (and the higher-order Gaussian modes detailed below) are solutions to the wave equation for an electromagnetic field in free space or in a homogeneous dielectric medium, obtained by combining Maxwell's equations for the curl of Template:Mvar and the curl of Template:Mvar, resulting in: $${\mathrm{\nabla }}^{2}U=\frac{1}{c^2}\frac{{\partial }^{2}U}{\partial t^2},$$ where Template:Mvar is the speed of light in the medium, and Template:Mvar could either refer to the electric or magnetic field vector, as any specific solution for either determines the other. The Gaussian beam solution is valid only in the paraxial approximation, that is, where wave propagation is limited to directions within a small angle of an axis. Without loss of generality let us take that direction to be the +z direction in which case the solution Template:Mvar can generally be written in terms of Template:Mvar which has no time dependence and varies relatively smoothly in space, with the main variation spatially corresponding to the wavenumber Template:Mvar in the Template:Mvar direction: $$U(x,y,z,t)=u(x,y,z)e^{-i(kz-\omega t)}\widehat{\mathbf{𝐱}}.$$

Using this form along with the paraxial approximation, ∂²u/∂z² can then be essentially neglected. Since solutions of the electromagnetic wave equation only hold for polarizations which are orthogonal to the direction of propagation (Template:Mvar), we have without loss of generality considered the polarization to be in the Template:Mvar direction so that we now solve a scalar equation for u(x, y, z).

Substituting this solution into the wave equation above yields the paraxial approximation to the scalar wave equation: $$\frac{{\partial }^{2}u}{\partial x^2}+\frac{{\partial }^{2}u}{\partial y^2}=2ik\frac{\partial u}{\partial z}.$$ Writing the wave equations in the light-cone coordinates returns this equation without utilizing any approximation. Gaussian beams of any beam waist w₀ satisfy the paraxial approximation to the scalar wave equation; this is most easily verified by expressing the wave at Template:Mvar in terms of the complex beam parameter q(z) as defined above. There are many other solutions. As solutions to a linear system, any combination of solutions (using addition or multiplication by a constant) is also a solution. The fundamental Gaussian happens to be the one that minimizes the product of minimum spot size and far-field divergence, as noted above. In seeking paraxial solutions, and in particular ones that would describe laser radiation that is not in the fundamental Gaussian mode, we will look for families of solutions with gradually increasing products of their divergences and minimum spot sizes. Two important orthogonal decompositions of this sort are the Hermite–Gaussian or Laguerre-Gaussian modes, corresponding to rectangular and circular symmetry respectively, as detailed in the next section. With both of these, the fundamental Gaussian beam we have been considering is the lowest order mode.

Higher-order modes

Hermite-Gaussian modes

File:Hermite-gaussian.png

Twelve Hermite-Gaussian modes

It is possible to decompose a coherent paraxial beam using the orthogonal set of so-called Hermite-Gaussian modes, any of which are given by the product of a factor in Template:Mvar and a factor in Template:Mvar. Such a solution is possible due to the separability in Template:Mvar and Template:Mvar in the paraxial Helmholtz equation as written in Cartesian coordinates. Thus given a mode of order (l, m) referring to the Template:Mvar and Template:Mvar directions, the electric field amplitude at x, y, z may be given by: $$E(x,y,z)=u_l(x,z)u_m(y,z)\exp (-ikz),$$ where the factors for the Template:Mvar and Template:Mvar dependence are each given by: $$u_J(x,z)={\left(\frac{\sqrt{2/\pi }}{2^{J}J!w_0}\right)}^{1/2}{\left(\frac{q_0}{q(z)}\right)}^{1/2}{(-\frac{q^{\ast }(z)}{q(z)})}^{J/2}{H}_J\left(\frac{\sqrt{2}x}{w(z)}\right)\exp (-i\frac{k{x}^2}{2q(z)}),$$ where we have employed the complex beam parameter q(z) (as defined above) for a beam of waist w₀ at Template:Mvar from the focus. In this form, the first factor is just a normalizing constant to make the set of u_J orthonormal. The second factor is an additional normalization dependent on Template:Mvar which compensates for the expansion of the spatial extent of the mode according to w(z)/w₀ (due to the last two factors). It also contains part of the Gouy phase. The third factor is a pure phase which enhances the Gouy phase shift for higher orders Template:Mvar.

The final two factors account for the spatial variation over Template:Mvar (or Template:Mvar). The fourth factor is the Hermite polynomial of order Template:Mvar ("physicists' form", i.e. H₁(x) = 2x), while the fifth accounts for the Gaussian amplitude fall-off exp(−x²/w(z)²), although this isn't obvious using the complex Template:Mvar in the exponent. Expansion of that exponential also produces a phase factor in Template:Mvar which accounts for the wavefront curvature (1/R(z)) at Template:Mvar along the beam.

Hermite-Gaussian modes are typically designated "TEM_lm"; the fundamental Gaussian beam may thus be referred to as TEM₀₀ (where TEM is transverse electro-magnetic). Multiplying u_l(x, z) and u_m(y, z) to get the 2-D mode profile, and removing the normalization so that the leading factor is just called E₀, we can write the (l, m) mode in the more accessible form:

$$\begin{array}{rl}{E}_{l,m}(x,y,z)=& E_0\frac{w_0}{w(z)}{H}_l\left(\frac{\sqrt{2}x}{w(z)}\right)H_m\left(\frac{\sqrt{2}y}{w(z)}\right)\times \exp \left(-\frac{x^2+y^2}{w^2(z)}\right)\exp \left(-i\frac{k(x^2+y^2)}{2R(z)}\right)\times \exp (i\psi (z))\exp (-ikz).\end{array}$$

In this form, the parameter w₀, as before, determines the family of modes, in particular scaling the spatial extent of the fundamental mode's waist and all other mode patterns at z = 0. Given that w₀, w(z) and R(z) have the same definitions as for the fundamental Gaussian beam described above. It can be seen that with l = m = 0 we obtain the fundamental Gaussian beam described earlier (since H₀ = 1). The only specific difference in the Template:Mvar and Template:Mvar profiles at any Template:Mvar are due to the Hermite polynomial factors for the order numbers Template:Mvar and Template:Mvar. However, there is a change in the evolution of the modes' Gouy phase over Template:Mvar: $$\psi (z)=(N+1)\arctan \left(\frac{z}{z_{\mathrm{R}}}\right),$$

where the combined order of the mode Template:Mvar is defined as N = l + m. While the Gouy phase shift for the fundamental (0,0) Gaussian mode only changes by ±π/2 radians over all of Template:Mvar (and only by ±π/4 radians between ±z_R), this is increased by the factor N + 1 for the higher order modes.

Hermite Gaussian modes, with their rectangular symmetry, are especially suited for the modal analysis of radiation from lasers whose cavity design is asymmetric in a rectangular fashion. On the other hand, lasers and systems with circular symmetry can better be handled using the set of Laguerre-Gaussian modes introduced in the next section.

Laguerre-Gaussian modes

File:Intensity profiles of Laguerre-Gaussian modes.pdf

Intensity profiles of the first 12 Laguerre-Gaussian modes.

Beam profiles which are circularly symmetric (or lasers with cavities that are cylindrically symmetric) are often best solved using the Laguerre-Gaussian modal decomposition. These functions are written in cylindrical coordinates using generalized Laguerre polynomials. Each transverse mode is again labelled using two integers, in this case the radial index p ≥ 0 and the azimuthal index Template:Mvar which can be positive or negative (or zero):

File:Focused Laguerre-Gaussian beam.webm

A Laguerre-Gaussian beam with l=1 and p=0. Red and blue indicate intensity of the electric field with positive and negative phase.

$$\begin{array}{rl}u(r,\varphi ,z)=& C_{lp}^{LG}\frac{1}{w(z)}{\left(\frac{r\sqrt{2}}{w(z)}\right)}^{|l|}\exp (-\frac{r^2}{w^2(z)})L_p^{|l|}\left(\frac{2r^2}{w^2(z)}\right)\times \\ & \exp (-ik\frac{r^2}{2R(z)})\exp (-il\varphi )\exp (i\psi (z)),\end{array}$$

where L_p^l are the generalized Laguerre polynomials. C is a required normalization constant: $$C_{lp}^{LG}=\sqrt{\frac{2p!}{\pi (p+|l|)!}}\Rightarrow \underset{0}{\overset{2\pi }{\int }}d\varphi \underset{0}{\overset{\mathrm{\infty }}{\int }}drr|u(r,\varphi ,z){|}^2=1,$$.

w(z) and R(z) have the same definitions as above. As with the higher-order Hermite-Gaussian modes the magnitude of the Laguerre-Gaussian modes' Gouy phase shift is exaggerated by the factor N + 1: $$\psi (z)=(N+1)\arctan \left(\frac{z}{z_{\mathrm{R}}}\right),$$ where in this case the combined mode number N = Template:Mabs + 2p. As before, the transverse amplitude variations are contained in the last two factors on the upper line of the equation, which again includes the basic Gaussian drop off in Template:Mvar but now multiplied by a Laguerre polynomial. The effect of the rotational mode number Template:Mvar, in addition to affecting the Laguerre polynomial, is mainly contained in the phase factor exp(−ilφ), in which the beam profile is advanced (or retarded) by Template:Mvar complete 2π phases in one rotation around the beam (in Template:Mvar). This is an example of an optical vortex of topological charge Template:Mvar, and can be associated with the orbital angular momentum of light in that mode.

Ince-Gaussian modes

File:Ince Gaussian Modes.jpg

Transverse amplitude profile of the lowest order even Ince-Gaussian modes.

In elliptic coordinates, one can write the higher-order modes using Ince polynomials. The even and odd Ince-Gaussian modes are given by

$$u_{\epsilon }(\xi ,\eta ,z)=\frac{w_0}{w\left(z\right)}{\mathrm{C}}_p^m(i\xi ,\epsilon ){\mathrm{C}}_p^m(\eta ,\epsilon )\exp [-ik\frac{r^2}{2q\left(z\right)}-(p+1)\zeta \left(z\right)],$$ where Template:Mvar and Template:Mvar are the radial and angular elliptic coordinates defined by $$\begin{array}{rl}x& =\sqrt{\epsilon /2}w(z)\cosh \xi \cos \eta ,\\ y& =\sqrt{\epsilon /2}w(z)\sinh \xi \sin \eta .\end{array}$$ C(η, ε) are the even Ince polynomials of order Template:Mvar and degree Template:Mvar where Template:Mvar is the ellipticity parameter. The Hermite-Gaussian and Laguerre-Gaussian modes are a special case of the Ince-Gaussian modes for ε = ∞ and ε = 0 respectively.

Hypergeometric-Gaussian modes

There is another important class of paraxial wave modes in cylindrical coordinates in which the complex amplitude is proportional to a confluent hypergeometric function.

These modes have a singular phase profile and are eigenfunctions of the photon orbital angular momentum. Their intensity profiles are characterized by a single brilliant ring; like Laguerre–Gaussian modes, their intensities fall to zero at the center (on the optical axis) except for the fundamental (0,0) mode. A mode's complex amplitude can be written in terms of the normalized (dimensionless) radial coordinate ρ = r/w₀ and the normalized longitudinal coordinate Ζ = z/z_R as follows:

$$\begin{array}{rl}{u}_{\mathsf{p}m}(\rho ,\varphi ,\mathrm{Z})=& \sqrt{\frac{2^{\mathsf{p}+|m|+1}}{\pi \mathrm{\Gamma }(\mathsf{p}+|m|+1)}}\frac{\mathrm{\Gamma }(\frac{\mathsf{p}}{2}+|m|+1)}{\mathrm{\Gamma }(|m|+1)}{i}^{|m|+1}\times \\ & {\mathrm{Z}}^{\frac{\mathsf{p}}{2}}(\mathrm{Z}+i{)}^{-(\frac{\mathsf{p}}{2}+|m|+1)}{\rho }^{|m|}\times \\ & \exp (-\frac{i{\rho }^2}{\mathrm{Z}+i})e^{im\varphi }{}_1{F}_1(-\frac{\mathsf{p}}{2},|m|+1;\frac{{\rho }^2}{\mathrm{Z}(\mathrm{Z}+i)})\end{array}$$

where the rotational index Template:Mvar is an integer, and $\mathsf{p}\ge -|m|$ is real-valued, Γ(x) is the gamma function and ₁F₁(a, b; x) is a confluent hypergeometric function.

Some subfamilies of hypergeometric-Gaussian (HyGG) modes can be listed as the modified Bessel-Gaussian modes, the modified exponential Gaussian modes, and the modified Laguerre–Gaussian modes.

The set of hypergeometric-Gaussian modes is overcomplete and is not an orthogonal set of modes. In spite of its complicated field profile, HyGG modes have a very simple profile at the beam waist (z = 0): $$u(\rho ,\varphi ,0)\propto {\rho }^{\mathsf{p}+|m|}{e}^{-{\rho }^2+im\varphi }.$$

See also

• Bessel beam
• Tophat beam
• Laser beam profiler
• Quasioptics

References

• Chapter 5, "Optical Beams," pp. 267.
• Chapter 3, "Beam Optics," pp. 80–107.
• Chapter 16.

External links

• Gaussian Beam Optics Tutorial, Newport