Gaussian beam

Intensity of a Gaussian beam around focus at an instant of time, showing two intensity peaks for each wavefront.

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.

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

In optics, a Gaussian beam is a beam of monochromatic electromagnetic radiation whose transverse magnetic and electric field amplitude profiles are given by the Gaussian function; this also implies a Gaussian intensity (irradiance) profile. This fundamental (or TEM₀₀) transverse gaussian mode describes the intended output of most (but not all) lasers, as such a beam can be focused into the most concentrated spot. When such a beam is refocused by a lens, the transverse phase dependence is altered; this results in a different Gaussian beam. The electric and magnetic field amplitude profiles along any such circular Gaussian beam (for a given wavelength and polarization) are determined by a single parameter: the so-called waist w₀. At any position z relative to the waist (focus) along a beam having a specified w₀, the field amplitudes and phases are thereby determined^[1] as detailed below.

The equations below assume a beam with a circular cross-section at all values of z; this can be seen by noting that a single transverse dimension, r, appears. Beams with elliptical cross-sections, or with waists at different positions in z 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 x and y.

Arbitrary solutions of the paraxial Helmholtz equation can be expressed as combinations of Hermite–Gaussian modes (whose amplitude profiles are separable in x and y using Cartesian coordinates) or similarly as combinations of Laguerre–Gaussian modes (whose amplitude profiles are separable in r and θ using cylindrical coordinates).^[2]^[3] At any point along the beam z 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 z, whereas the propagation of any single Hermite–Gaussian (or Laguerre–Gaussian) mode retains the same form along a beam.

Although there are other possible modal decompositions, these families of solutions are the most 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.

Mathematical form

The Gaussian beam is a transverse electromagnetic (TEM) mode.^[4] The mathematical expression for the electric field amplitude is a solution to the paraxial Helmholtz equation.^[1] Assuming polarization in the x direction and propagation in the +z direction, the electric field in phasor (complex) notation is given by:

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

where^[1]

r

is the radial distance from the center axis of the beam,

z

is the axial distance from the beam's focus (or "waist"),

i

is the imaginary unit,

k = 2 \pi/\lambda

is the wave number (in radians per meter) for a wavelength λ,

E_0 = E(0,0)

, the electric field amplitude (and phase) at the origin at time 0,

w(z)

is the radius at which the field amplitudes fall to 1/e of their axial values, at the plane z along the beam,

w_0 = w(0)

is the waist size,

R(z)

is the radius of curvature of the beam's wavefronts at z, and

\psi(z)

is the Gouy phase at z, an extra phase term beyond that attributable to the phase velocity of light.

There is also an understood time dependence $e^{i\omega t}$ multiplying such phasor quantities; the actual field at a point in time and space is given by the real part of that complex quantity.

The wave's magnetic field has an identical form but with an orthogonal polarization (in y since the electric field polarization was stipulated to be in x):

{\mathbf H(r,z)} = \hat{y} \frac{1}{\eta} {E_x(r,z)}

where the constant η is the characteristic impedance of the medium in which the beam is propagating. For free space, η = η₀ ≈ 377 Ω.

The time-averaged intensity (or irradiance) at a location is computed using $I = \frac{1}{2} \mathbf{Re}(E \times H^*)$ which removes all phase factors (since we've averaged over time, which also results in the ½ factor):

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

where $I_0 = E_0^2/2 \eta$ is the intensity at the center of the beam at its waist.

Evolving beam width

At a position z along the beam (measured from the focus), the spot size parameter w is given by^[1]

w(z) = w_0 \, \sqrt{ 1+ {\left( \frac{z}{z_\mathrm{R}} \right)}^2 } \ .

where^[1]

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

is called the Rayleigh range as further discussed below.

Evolving radius of curvature

The curvature of the wavefronts is zero at the beam waist and also approaches zero as z → ±∞. It is equal to 1/R where R(z) is the radius of curvature as a function of position along the beam, given by^[1]

R(z) = z \left[{ 1+ {\left( \frac{z_\mathrm{R}}{z} \right)}^2 } \right] \ .

Gouy phase

The so-called Gouy phase of the beam at z is given by:^[1]

\psi(z) = \arctan \left( \frac{z}{z_\mathrm{R}} \right) \ .

The Gouy phase results in an increase in the apparent wavelength near the waist. The phase velocity near the waist exceeds the speed of light in the medium, just as it can in a waveguide. The Gouy phase shift along the beam remains within the range ±π/2 (for a fundamental Gaussian beam) and is not observable in most experiments. However it is of theoretical importance and takes on a greater range for higher-order Gaussian modes.^[5]

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 x and y 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.

Beam parameters

The geometric dependence of the fields of a Gaussian beam are governed by the light's wavelength λ (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

Rayleigh range and confocal parameter

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

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

At a distance from the waist equal to the Rayleigh range z_R, the width w of the beam is $\sqrt{2}$ 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.^[1]

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, let us call the "edge" of a beam the radius where r = w(z). That is where the intensity has dropped to 1/e² of its on-axis value. Now, for $z \gg z_\mathrm{R}$ the parameter $w(z)$ increases linearly with $z$ . This means that far from the waist, the beam "edge" (in the above sense) is cone-shaped. The angle between lines along that cone (whose $r=w(z)$ ) and the central axis of the beam ( $r=0$ ) is called the divergence of the beam. It is given by^[1]

\theta \simeq \frac{\lambda}{\pi w_0} \qquad (\theta \mathrm{\ in\ radians}).

The total angular spread of the beam far from the waist is then given by

\Theta = 2 \theta\ .

Because the divergence is inversely proportional to the spot size, for a given wavelength λ, 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 crossection (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.^[6] From the above expression for divergence, this means the Gaussian beam model is only accurate for beams with waists larger than about $2\lambda/\pi$ .

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 $w_0$ . 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 $\mathrm{NA} = n \sin \theta$ , where n 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} = w_0 / \mathrm{NA}

Power and intensity

Power through an aperture

The power P passing through a circle of radius r in the transverse plane at position z is^[7]

P(r,z) = P_0 \left[ 1 - e^{-2r^2 / w^2(z)} \right]\ ,

where

P_0 = { 1 \over 2 } \pi I_0 w_0^2

is the total power transmitted by the beam.

For a circle of radius $r = w(z) \,$ , the fraction of power transmitted through the circle is

{ P(z) \over P_0 } = 1 - e^{-2} \approx 0.865\ .

Similarly, about 90 percent of the beam's power will flow through a circle of radius $r = 1.07\cdot w(z)$ , 95 percent through a circle of radius $r = 1.224\cdot w(z)$ , and 99 percent through a circle of radius $r = 1.52\cdot w(z)$ .^[7]

Peak intensity

The peak intensity at an axial distance $z$ from the beam waist can be calculated as the limit of the enclosed power within a circle of radius $r$ , divided by the area of the circle $\pi r^2$ as the circle shrinks:

I(0,z) =\lim_{r\to 0} \frac {P_0 \left[ 1 - e^{-2r^2 / w^2(z)} \right]} {\pi r^2}

The limit can be evaluated using L'Hôpital's rule:

I(0,z) = \frac{P_0}{\pi} \lim_{r\to 0} \frac { \left[ -(-2)(2r) e^{-2r^2 / w^2(z)} \right]} {w^2(z)(2r)} = {2P_0 \over \pi w^2(z)}.

Complex beam parameter

Main article: Complex beam parameter

The spot size and curvature of a Gaussian beam as a function of z along the beam can also be encoded in the complex beam parameter $q(z)$ ^[8]^[9] given by:

q(z) = z + iz_\mathrm{R} \ .

Introducing this complication leads to a simplification of the Gaussian beam field equation as shown below. It can be seen that the reciprocal of q(z) contains the wavefront curvature and relative on-axis intensity in its real and imaginary parts, respectively:^[8]

{ 1 \over q(z) } = { 1 \over z + iz_\mathrm{R} } = { z \over z^2 + z_\mathrm{R}^2 } - i { z_\mathrm{R} \over z^2 + z_\mathrm{R}^2 } = {1 \over R(z) } - i { \lambda \over \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 u the relative field strength of an elliptical Gaussian beam (with the elliptical axes in the x and y directions) then it can be separated in x and y according to:

{u}(x,y,z) = {u_x}(x,z)\, {u_y}(y,z),

where

{u_x}(x,z) = \frac{1}{\sqrt{{q}_x(z)}} \exp\left(-i k \frac{x^2}{2 {q}_x(z)}\right)

{u_y}(y,z) = \frac{1}{\sqrt{{q}_y(z)}} \exp\left(-i k \frac{y^2}{2 {q}_y(z)}\right)

where $q_x(z)$ and $q_y(z)$ are the complex beam parameters in the x and y directions.

For the common case of a circular beam profile, ${q}_x = {q}_y = {q}$ and $x^2 + y^2 = r^2$ , which yields^[10]

{u}(r,z) = \frac{1}{{q}(z)}\exp\left( -i k\frac{r^2}{2 {q}(z)}\right).

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:^[11] obtained by combining Maxwell's equations for the curl of E and the curl of H, resulting in:

\nabla^2 U = \frac{1}{c^2} \frac{\partial^2 U}{\partial t^2},

where c is the speed of light in the medium, and $U$ 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 U can generally be written in terms of u which has no time dependence and varies relatively smoothly in space, with the main variation spatially corresponding to the wavenumber k in the z direction:^[11]

U(x,y,z,t) = u(x,y,z) e^{-i(kz-\omega t)} \, \hat{x} \; .

Using this form along with the paraxial approximation, $\partial^2 u/\partial z^2$ can then be essentially neglected. Since solutions of the electromagnetic wave equation only hold for polarizations which are orthogonal to the direction of propagation (z), we have without loss of generality considered the polarization to be in the x 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:^[11]

\frac{\partial^2 u}{\partial x^2} + \frac{\partial^2 u}{\partial y^2} = 2ik \frac{\partial u}{\partial z}.

Gaussian mode solution

It can be verified that Gaussian beams of any beam waist w₀ satisfy this wave equation; this is most easily accomplished by expressing the wave at z in terms of the complex beam parameter q(z) as defined above.

Twice differentiating that expression for u(r,z) (where r² = x² + y²) with respect to x yields:

\frac{\partial^2 u}{\partial x^2} \; = \; u \left (- \frac{ik}{q} + \left ( \frac{-ikx}{q} \right )^2 \right ) \; = \; u \left (- \frac{ik}{q} - \frac{k^2 x^2}{q^2} \right )

and likewise for y. Forming the sum in the left hand side of the above scalar wave equation then yields:

\frac{\partial^2 u}{\partial x^2} + \frac{\partial^2 u}{\partial y^2} \; = \; u \left (- 2\frac{ik}{q} - \frac{k^2 r^2}{q^2} \right )

Now differentiating u with respect to z, we find:

\frac{\partial^2 u}{\partial z^2} \; = \; u \left (- \frac{1}{q} + \frac{-ikr^2}{2q^2} \right ) \;

from which the right hand side of the wave equation is found to be:

2ik \frac{\partial^2 u}{\partial z^2} \; = \; u \left (- \frac{2ik}{q} - \frac{k^2 r^2}{q^2} \right ) \;

identical to the above result for the left hand side.

Higher-order modes

Hermite-Gaussian modes

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 is given by the product of a factor in x and a factor in y. Such a solution is possible due to the separability in x and y in the paraxial Helmholtz equation as written in Cartesian coordinates.^[12] Thus given a mode of order (l,m) referring to the x and y directions, the electric field amplitude at x,y,z may be given by: $E(x,y,z) = u_l(x,z) u_m(y,z)$ where the factors for the x and y dependence are each given by:

${u}_J(x,z) = \left(\frac{\sqrt{2/\pi}}{ 2^J \; J! \; w_0}\right)^{\!\!1/2} \!\! \left( \frac{{q}_0}{{q}(z)}\right)^{\!\!1/2} \!\! \left(- \frac{{q}^\ast(z)}{{q}(z)}\right)^{\!\! J/2} \!\! H_J\left(\frac{\sqrt{2}x}{w(z)}\right) \, \exp \! \left(\! -i \frac{k x^2}{2 {q}(z)}\right)$

where we have employed the complex beam parameter q(z) (as defined above) for a beam of waist w₀ at z 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 z 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 J.

The final two factors account for the spatial variation over x (or y). The fourth factor is the Hermite polynomial of order $J$ ("physicists' form", i.e. $H_1(x)=2x\,$ ), while the fifth accounts for the Gaussian amplitude fall-off $\exp(-x^2/w(z)^2)$ , although this isn't obvious using the complex q in the exponent. Expansion of that exponential also produces a phase factor in x which accounts for the wavefront curvature (1/R(z)) at z along the beam.

Hermite-Gaussian modes are typically designated "TEM_lm"; the fundamental Gaussian beam may thus be referred to as TEM₀₀ (where TEM stands for 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: $E_{l,m} (x,y,z) = E_0 \frac{w_0}{w(z)} \!\ H_l \! \! \left(\frac{\sqrt{2} \,x}{w(z)}\right) \! H_m \! \! \left(\frac{\sqrt{2} \, y}{w(z)}\right) \, \exp \! \! \left( \! -\frac{x^2+y^2}{w^2(z)} \right) \times$

\exp \! \left( \! -i\frac{k(x^2+y^2)}{2R(z)} \right) \exp ( \! -ikz) \exp ( i \psi(z)) \; \;

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 x and y profiles at any z are due to the Hermite polynomial factors for the order numbers l and m. However there is a change in the evolution of the modes' Gouy phase over z:

\psi(z) = (N+1) \, \arctan \left( \frac{z}{z_\mathrm{R}} \right)

where the combined order of the mode N 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 z (and only by ±π/4 radians between ±Z_R), this is increased by the factor N+1 for the higher order modes.^[5]

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 Lageurre-Gaussian modes introduced in the next section.

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.^[3] These functions are written in cylindrical coordinates using Laguerre polynomials. Each transverse mode is again labelled using two integers, in this case the radial index $p\ge 0$ and the azimuthal index $l$ which can be positive or negative (or zero).

{u}(r,\phi,z)=\frac{C^{LG}_{lp}}{w(z)}\left(\frac{r \sqrt{2}}{w(z)}\right)^{\! |l|} \exp\! \left(\! -\frac{r^2}{w^2(z)}\right)L_p^{|l|} \! \left(\frac{2r^2}{w^2(z)}\right) \times

\exp \! \left(\! - i k \frac{r^2}{2 R(z)}\right) \exp(i l \phi) \, \exp ( \! -ikz) \, \exp(i \psi(z)) \; \;

^[13]

where $L_p^l$ are the generalized Laguerre polynomials. $C^{LG}_{lp}$ is a required normalization constant not detailed here; $w(z)$ 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 exagerated 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 = |l| + 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 r but now multiplied by a Laguerre polynomial. The effect of the rotational mode number l, 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 l complete 2π phases in one rotation around the beam (in φ). This is an example of an optical vortex of topological charge l, and can be associated with the orbital angular momentum of light in that mode.

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 ^[14]

u_\varepsilon \left( \xi ,\eta ,z\right) = \frac{w_{0}}{w\left( z\right) }\mathrm{C}_{p}^{m}\left( i\xi ,\varepsilon \right) \mathrm{C} _{p}^{m}\left( \eta ,\varepsilon \right) \exp \left[ -ik\frac{r^{2}}{ 2q\left( z\right) }-\left( p+1\right) \zeta\left( z\right) \right] ,

where $\xi$ and $\eta$ are the radial and angular elliptic coordinates defined by

x = \sqrt{\varepsilon /2}w\left( z\right) \cosh \xi \cos \eta ,

y = \sqrt{\varepsilon /2}w\left( z\right) \sinh \xi \sin \eta.

${C}_{p}^{m}\left( \eta ,\varepsilon \right)$ are the even Ince polynomials of order $p$ and degree $m$ where $\varepsilon$ is the ellipticity parameter. The Hermite-Gaussian and Laguerre-Gaussian modes are a special case of the Ince-Gaussian modes for $\varepsilon=\infty$ and $\varepsilon=0$ 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 $\rho=r/w_0$ and the normalized longitudinal coordinate $\Zeta=z/z_R$ .^[15] as follows:

u_{{\mathsf p}m}(\rho,\theta,\Zeta)= \sqrt{\frac{2^{{\mathsf p}+|m|+1}}{\pi\Gamma({\mathsf p}+|m|+1)}} \; \frac{\Gamma(1+|m|+\frac{{\mathsf p}}{2})}{\Gamma(|m|+1)} \,\,i^{|m|+1} \; \; \cdot

\Zeta^{\frac{{\mathsf p}}{2}} \; (\Zeta+i)^{-(1+|m|+\frac{{\mathsf p}}{2})} \; \rho^{|m|} \; \; \cdot

\exp\left(-\frac{i\rho^2}{(\Zeta+i)}\right) \; e^{im\phi} \; {}_{1}F_{1}\left(-\frac{{\mathsf p}}{2}, |m|+1;\frac{r^2}{\Zeta(\Zeta+i)}\right)

where the rotational index $m$ is an integer, and ${\mathsf p}\ge-|m|$ is real valued, $\Gamma(x)$ is the gamma function and ${}_{1}F_{1}(a,b;x)$ 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 pupil plane ( $\Zeta=0$ ):

u(\rho,\phi,0) \propto \rho^{{\mathsf p}+|m|}e^{-\rho^2+im\phi}.

See Optical vortex, which explains that the outcoming wave from a pitch-fork hologram is a sub-family of HyGG modes. The HyGG profile while beam propagates along $\zeta$ has a dramatic change and it is not a stable mode below the Rayleigh range.

Notes

1 2 3 4 5 6 7 8 9 Svelto, pp. 153–5.
↑ Siegman, p. 642.
1 2 probably first considered by Goubau and Schwering (1961).
↑ Svelto, p. 158.
1 2 Paschotta, Rüdiger. "Gouy Phase Shift". Encyclopedia of Laser Physics and Technology. RP Photonics. Retrieved May 2, 2014.
↑ Siegman (1986) p. 630.
1 2 Melles Griot. Gaussian Beam Optics
1 2 Siegman, pp. 638–40.
↑ Garg, pp. 165–168.
↑ See Siegman (1986) p. 639. Eq. 29
1 2 3 Svelto, pp. 148–9.
↑ Siegman (1986), p645, eq. 54
↑ Allen, L. (June 1, 1992). "Orbital angular momentum of light and the transformation of Laguerre-Gaussian laser modes" (PDF). Physical Review A 45 (11): 8185. Bibcode:1992PhRvA..45.8185A. doi:10.1103/physreva.45.8185.
↑ Bandres and Gutierrez-Vega (2004)
↑ Karimi et. al (2007)

References

Bandres, Miguel A.; Gutierrez-Vega, Julio C. (2004). "Ince Gaussian beams". Opt. Lett. (OSA) 29 (2): 144–146. Bibcode:2004OptL...29..144B. doi:10.1364/OL.29.000144. PMID 14743992.
Garg, Anupam (2012). Classical Electromagnetism in a Nutshell. Princeton, N.J.: Princeton University Press. ISBN 0691130183.
Goubau, G. and Schwering, F. (1961). "On the guided propagation of electromagnetic wave beams". IRE Trans. 9: 248–256. Bibcode:1961ITAP....9..248G. doi:10.1109/TAP.1961.1144999. MR 0134166.
Karimi, E.; Zito, G.; Piccirillo, B.; Marrucci, L.; Santamato, E. (2007). "Hypergeometric-Gaussian beams". Opt. Lett. (OSA) 32 (21): 3053–3055. arXiv:0712.0782. Bibcode:2007OptL...32.3053K. doi:10.1364/OL.32.003053. PMID 17975594.
Mandel, Leonard; Wolf, Emil (1995). Optical Coherence and Quantum Optics. Cambridge: Cambridge University Press. ISBN 0-521-41711-2. Chapter 5, "Optical Beams," pp. 267.
Pampaloni,F. and Enderlein, J. (2004). "Gaussian, Hermite-Gaussian, and Laguerre-Gaussian beams: A primer". arXiv:physics/0410021 [physics.optics].
Saleh, Bahaa E. A.; Teich, Malvin Carl (1991). Fundamentals of Photonics. New York: John Wiley & Sons. ISBN 0-471-83965-5. Chapter 3, "Beam Optics," pp. 80–107.
Siegman, Anthony E. (1986). Lasers. University Science Books. ISBN 0-935702-11-3. Chapter 16.
Svelto, Orazio (2010). Principles of Lasers (5th ed.).
Yariv, Amnon (1989). Quantum Electronics (3rd ed.). Wiley. ISBN 0-471-60997-8.

External links

Gaussian Beam Propagation - IDEX Optics & Photonics Technical Guide
Gaussian Beam Optics Tutorial, Newport

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