Since their introduction 60 years ago,1 lasers with various characteristics have developed rapidly, making them important light sources in various fields ranging from scientific research2^–4 to industrial production.5^–8 Almost all the characteristics of a laser can be classified as temporal,9^–14 spatial,15^–18 or spectral domain.19^–23 Over the past few decades, much interest has been given to laser properties in the temporal and spectral domains, while the spatial properties of laser beams seem to be relatively less emphasized. In the last 10 to 20 years, as a result of the emergence of research on spatial characteristics of laser beams, especially, the orbital angular momentum (OAM), much more attention has been paid to structured laser beams with distinct spatial or spatiotemporal structures. Such beams have brought various breakthroughs to many fields, including imaging,24^,25 microscopy,26^,27 metrology,28^–30 communication,31^–33 optical trapping,34^–36 and quantum information processing.37^–39 In the most recent five years, the number of reviews on structured light has boomed, with the majority of reviews focusing on technical-level research into the phenomenon,40^–54 such as the generation and detection technology of structured light,44^,45 application in the field of optical trapping46^,47 and anti-turbulence,48 progress in optical vortices49^–51 and higher-dimensional structured light,52 as well as research on structured light in flat optics53 and nonlinear optics.54 In contrast, there have been few studies on the evolution of the investigations and corresponding understandings of the pattern formation of structured laser beams. Here, we would like to take the spatial patterns as the main core to review the evolution and recent advancement on spatial patterns of structured laser beams, from the early spontaneous organization with numerical solutions of mathematical equations and eigenmode superposition theories to the multiple transformations of the spatiotemporal dimensions and nonlinear process of structured laser beams.

The research on spatial patterns of structured laser beams went through two periods: the first was the spontaneous organization of patterns described by relative equations, while the second was the transformation of laser patterns on demand. Although there is no distinct separation between these two periods, it is noticeable that over the past 10 years, we have steadily gained a better understanding of how diverse laser spatial patterns originate and developed several effective techniques for producing spatial patterns on demand. Research on the formation of structured laser patterns was a main focus in physics from the 1960s to 1990s.55^–69 The earliest research at that time combined Maxwell’s equations69 with Schrödinger’s equation,70 leading to the laser amplitude $E$ coupled with the collective variables $P$ and $D$ for the atomic polarization and population inversion to describe the transverse mode formation.71 This set of equations is called the MB equations.62^,72 Then, on the basis of the MB equations, which are a set of spatiotemporal multivariate nonlinear partial differential equations, the pattern formation characteristics of class A, B, and C lasers were successively studied.68^,71 The relevant equations are then further developed, and equations, such as the complex Ginzburg–Landau (CGL),73^,74 complex Swift–Hohenberg (CSH),75^,76 and Kuramoto–Sivashinsky (KS)77^–80 equations were further derived. Through the numerical solution of these equations, the formation of laser transverse patterns under specific parameters can be analyzed. In addition, with time and space terms involved, these equations can explain both the spatial and temporal characteristics of the patterns in some cases, including stability, oscillation, chaos, and so on.81^–83 However, most of these patterns are ideal cases obtained under the condition of a single transverse mode of the laser.62 If multiple transverse modes with different frequencies are involved, it would be hard to analyze the results of multifrequency interaction through these equations. Therefore, in the study of pattern formation in the last 20 years, the analysis is often carried out through the applications of a set of eigenmode superposition theories.84^–89 This set of theories mainly studies the spatial structure characteristics of the patterns. The basis of eigenmode superposition theory is the fundamental composed modes, such as Hermite–Gaussian (HG), Laguerre–Gaussian (LG), and Ince–Gaussian (IG) modes, obtained by solving the Helmholtz equations,90^–96 except with space terms and without time terms. Then, according to the specific laser cavity conditions and field distributions of the output pattern, it could be analyzed whether coherent or incoherent superposition of the fundamental modes is generated through the eigenmode superposition theory. This involves the concept of transverse mode locking (TML),97^–99 namely, to lock the phase100^,101 or frequency of several transverse modes to obtain the output beam. The cooperatively frequency-locked multimode regime, in which at least two transverse modes contribute significantly to the output field, lock to a common frequency with which they oscillate in a synchronized way. The locking concerns also the relative phases of the modes, so that the output intensity has a stationary transverse configuration. The patterns formed by the TML effect could possess phase singularities in dark points.102 The theory of eigenmode superposition can also explain the formation of high-order complex transverse modes and optical vortex lattices (OVLs).87^–89

For the second period of on-demand transformation of laser patterns, a number of techniques have been developed in the past 20 years to actively control the generation and transformation of laser beam patterns, giving rise to a better understanding of the spatial features of lasers. Numerous review articles on the actively controlled generation of structured laser patterns, using both intracavity oscillation40^,41 and extracavity spatial modulation methods, are readily available.42^–45 The studies on the transformations of structured laser beams are mostly under the premise of single longitudinal mode. However, if multiple longitudinal modes are involved, the time dimension is supposed to be reconsidered. Recently, research on spatiotemporal beams has sprung up.103^–114 The direct generation of spatiotemporal beams involves the principle of spatiotemporal mode locking, i.e., locking the laser longitudinal and transverse modes at the same time to form ultrashort pulses with special spatial intensity distribution.103 Spatiotemporal mode locking is often obtained in fiber lasers, which realizes TML with the help of spatial filtering,107^,115 and longitudinal mode locking with the help of normal-dispersion mode-locking principle116^,117 and a saturable absorber. The spatiotemporal mode-locking beam opens up a new direction for the propagation and application of nonlinear waves. However, the spatiotemporal mode-locking beams produced directly by fiber lasers often have irregular intensity distributions. To obtain regular and more complex spatiotemporal beams, a pulse shaper based on spatial light modulator (SLM) is applied, which can generate specific spatiotemporal optical vortices,118^–120 spatiotemporal Airy beams,121 spatiotemporal Bessel beams,122 and so on.123^–126 Another method for actively controlling the generation and transformation of structured laser beams is using nonlinear processes. Combining nonlinear frequency conversion with the generation of structured laser beams, the beam patterns of harmonic waves are found to be endowed with much richer spatial information. Through nonlinear frequency conversion of structured laser beams, the beam pattern transformations in sum frequency generation (SFG),127^–130 second-harmonic generation (SHG),131^–140 four-wave mixing (FWM),141^,142 and other frequency upconversion143^–145 processes are carried out. Usually, these studies first generate structured beams with the help of modulation devices (such as SLM), and then carry out nonlinear conversion, which belongs to the external cavity nonlinear process of structured laser beams. Meanwhile, for the intracavity nonlinear process of structured laser beams, some studies also showed similar properties, while more complex and diverse beam patterns can be obtained.146^–150

The timeline of the evolution on spatial patterns of structured laser beams is shown in Fig. 1. In this review, we highlight the developments in laser spatial pattern studies with the emphasis on the spontaneous organization of pattern formation and the multiple transformations of laser spatial patterns. The original descriptive equations in the field of pattern formation are introduced in Sec. 2, including MB, CGL, CSH, and KS equations, which are fundamental to understanding the dynamics of pattern formation. Then, the current theories in the past 20 years are further discussed in Sec. 3, namely, the eigenmode superposition theories. The superposition of transverse modes brings a new vision in understanding laser physics and recognizing the vast possibilities for structured laser beam patterns. Results are analyzed and compared, covering coherent superpositions and incoherent superpositions. Then, in Sec. 4, more potential developments are forecast in spatiotemporal laser beams, particularly in spatiotemporal mode locking in fiber lasers and spatiotemporal beams generated through pulse shapers based on SLM. In Sec. 5, various nonlinear processes of structured laser beams from external–cavity modulations to intracavity transformation are comprehensively reviewed. Finally, concluding remarks and prospects are provided in Sec. 6.

Pattern formation is a ubiquitous phenomenon in nature and a phenomenon often found in laboratories; it was regarded as the spontaneous appearance of spatial order.150 Generally, all the patterns have something in common: they appear in spatially expanding dissipative systems, which are far from equilibrium because of some external pressure. In optical systems, the mechanism of pattern formation is the interaction among diffraction, partial resonance excitation, and nonlinearity. Diffraction is responsible for spatial coupling, which is necessary for the existence of nonuniform distribution of light fields. The role of nonlinearity is to select a specific pattern from several possible patterns. After reducing a specific model into a simpler model, a common theoretical model describing pattern formation is found to be the order parametric equation (OPE).150^,151 Then, in the study of pattern formation in structured laser systems, the problem was precisely addressed through the description of optical resonators by OPE, which reflects the general characteristics of laser transverse patterns.

The exploration of the OPE of laser spatial pattern formation can be traced back to the 1970s.55^–57 By simplifying the laser equations for the class A case to the CGL equation, the relationship between superfluid and laser dynamics was established. In view of this common theoretical description, it was expected that the dynamics of pattern formation in lasers and the dynamics of superfluidity would show identical features.53 Then, in the late 1980s57^–60 and 1990s,61^–64^,66 the formation of optical transverse modes began to be an interesting topic for scientists in MB equation field theory.

It was found that if the Maxwell equations69 and the Schrödinger equation70 are coupled to constrain the $N$ atoms in the cavity and expand the field in the cavity mode, then the amplitude $E$ is coupled with atomic polarization $P$ and population $D$.71 The set of equations is called the MB equation system, which is also the earliest manifestation of passive systems.152 When extended to the laser system, the dynamic of the electromagnetic field in the cavity with a planar end mirror should be considered, and the planar end mirror accommodates two-energy-level atoms as an active medium. The form of the MB equation becomes62$$\{\begin{array}{l}\frac{\partial E}{\partial t}=-(i{\omega }_c+\kappa )E+\kappa P+id\kappa {\nabla }^{2}E\\ \frac{\partial P}{\partial t}=-{\gamma }_{\perp }P+{\gamma }_{\perp }ED\\ \frac{\partial D}{\partial t}=-{\gamma }_{\prod }[(D-D_0)+\frac{1}{2}(E^{*}P+P^{*}E)]\end{array},$$(1)where $E$ is the field amplitude; $P$ is the atomic polarization intensity; $D$ is the population intensity; $\kappa$, ${\gamma }_{\perp }$, and ${\gamma }_{\prod }$ are the corresponding relaxation rates; ${\omega }_c$ is the cavity resonance frequency; and $d$ is the diffraction coefficient. The system of Eq. (1) determines the behavior of the restricted electromagnetic field $E$ in the transverse plane, which explains the formation mechanism of the transverse mode at the atomic level. Here, $(x,y)$ is a plane perpendicular to the $z$ axis of the cavity, and it is assumed that $E$ and $P$ have the best plane wave dependence in the $z$ direction and the slow residual dependence on the lateral variables $x$ and $y$. They directly follow the Maxwell equations of the field $E$ together with the Bloch equations of complex atomic polarization $P$ and population $N$. Numerically solving the MB equations, the laser transverse patterns observed in solid-state lasers are shown in Figs. 2(a) and 2(b).

By observing the form of the MB Eq. (1), it can be found that they are similar to the Lorentz model describing hydrodynamic instability.154 The similarity between the Lorentz model and the MB equations implies that chaotic instability can happen in single-mode and homogeneous line lasers. However, the consideration of time scale excludes the complete dynamics of Eq. (1) in lasers. In the Lorentz model, the damping rates differ by 1 order of magnitude from each other. On the contrary, in most lasers, the three damping rates of the MB equations are different from each other. Then, according to the relationship among the three damping rates $\kappa$, ${\gamma }_{\perp }$, and ${\gamma }_{\prod }$, the MB equations can be transformed into different forms under specific laser conditions, which can describe both pattern formation and time-domain properties.71

For class A lasers (e.g., He–Ne, Ar, Kr, and dye): ${\gamma }_{\perp }\approx {\gamma }_{\prod }\gg \kappa$, the polarization and the population inversion of the atom can be adiabatically eliminated; hence the system is only described by one field equation. The equation can be simplified to the CGL equation, which is also the governing equation in superconductors and superfluids. Therefore, the last two equations of Eq. (1) are eliminated, leaving only the nonlinear equation representing the field amplitude $E$ as follows:74$$\frac{\partial E}{\partial \tau }=(D_0-1)E-i(\beta -d{\nabla }^2)E-g{(\beta -d{\nabla }^2)}^{2}E-E{|E|}^2,$$(2)where $\tau$ is the scaled time. Equation (2) retains all the ingredients of spatial pattern formation in lasers. One important property of the radiation in lasers is its diffraction, which is explained by the second term on the right-hand side of Eq. (2). The third term on the right-hand side of Eq. (2) describes the spatial frequency (transverse mode) selection, a phenomenon essential for the correct description of narrow-gain-line lasers. In many such lasers, the selection of transverse modes is possible by tuning the length of the resonator. Then, the first and last terms on the right-hand side of Eq. (2) give the normal form of a supercritical Hopf bifurcation. When the control parameter $D_0-1$ goes through zero, a bifurcation occurs, characterized by a fixed amplitude but an arbitrary phase.

For class B lasers (e.g., ruby, Nd, and ${\mathrm{CO}}_2$): ${\gamma }_{\perp }\gg {\gamma }_{\prod }\approx \kappa$, only the polarization intensity can be adiabatically eliminated. Then, its dynamic behavior is described by two coupled nonlinear equations corresponding to the light field and the population as follows:76$$\{\begin{array}{l}\frac{\partial E}{\partial \tau }=(D-1)E-i(\beta -d{\nabla }^2)E-g(\beta -d{\nabla }^2{)}^{2}E\\ \frac{\partial D}{\partial \tau }=-{\gamma }_{\prod }[(D-D_0)+|E{|}^{2}D]\end{array}.$$(3)

The first equation of Eq. (3) is the CSH dissipation equation suitable for class B lasers, where the higher-order diffusion term explains the choice of transverse modes. Comparing Eqs. (2) and (3), it can be found that in Eq. (3), the population $D$ is the recovery variable and the fast light field $E$ is the excitable variable. The overall particle inversion speed is slow, and the CSH equation contains additional nonlocal terms responsible for spatial mode selection, which will lead to the instability of pattern formation.

For class A and class B lasers, the output is stable in the absence of external disturbances. To realize an unstable operation, at least one degree of freedom needs to be added. The usual methods are as follows:155^–157 (1) modulate a certain parameter, such as the external field, pump rate, or cavity loss, to make the system a non-self-consistent equation system [Fig. 2(c)]; (2) inject the external field to increase the degrees of freedom of the system; (3) apply a two-way ring laser. In this case, the two backpropagating modes are coupled to each other, so that the number of degrees of freedom of the system is greater than two. Moreover, under the same conditions, observing the pattern formation of class B lasers will reveal two phenomena: periodic dynamics and low-dimensional deterministic chaos76 [Fig. 2(e)]. Accordingly, fixed patterns and weak turbulence are the characteristics of class A laser output patterns74 [Fig. 2(d)].

In addition, Huyet et al.77 used multi-scale expansion to derive the CSH equation of the laser. They obtained two fields’ equations: one is mainly caused by the phase fluctuations of the KS equation called the turbulent state,158 while the other CSH equation produces periodic modulation in spatial and temporal intensities. The reason that the laser intensity is locally chaotic is explained by this system of equations, while the time-averaged intensity pattern maintains the overall symmetry of the system. The time-domain dynamics of laser pattern formation were further studied by Chen and Lan.153^,159 The ring beam distributed pumping technology is used to obtain the high-order ${\mathrm{LG}}_{0,l}$ pattern. By slightly adjusting the spherical output coupling mirror, i.e., controlling the frequency difference $\mathrm{\Delta }\mathrm{\Omega }$ of the two ${\mathrm{LG}}_{0,l}$ patterns, the relationship between $\mathrm{\Delta }\mathrm{\Omega }$ and the relaxation oscillation frequency ${\omega }_r$ of the solid-state laser is constantly changing, accounting for the different time-domain properties [Fig. 2(f)].

In summary, the derivation and deformation of the MB equations have laid the physical foundation for the spontaneous organization of spatial patterns of structured laser beams. The formation of one-dimensional (1D) and two-dimensional (2D) spatial patterns can be explained by solving the MB equations and its modified CGL, CSH, and KS equations under specific conditions. In addition, since the MB equations are a system of multivariate nonlinear equations in space and time, the time-domain properties of certain cases in laser pattern formation, such as stability, oscillation, and chaos, can also be described.

Since structured laser beams often appear as time-averaged patterns in practical applications,76^,77^,86 their spatial characteristics have received much attention in recent years. Here, we should refer to the Helmholtz equation,90^–96 which is the basic wave equation that the electric vector of optical frequency electromagnetic field should satisfy under the scalar field approximation. Generally, both the Helmholtz equation and MB equations can describe the formation dynamics of laser spatial patterns, while the difference is that the former does not contain the temporal term, and the latter is a set of spatiotemporal equations. Hence, for the analysis of spatial characteristics of laser transverse patterns, it is more common to solve the Helmholtz equation, $${\nabla }^{2}E+k^{2}E=0,$$(4)where ${\nabla }^2$ is the Laplacian operator, $E$ refers to the light field, and $k=2\pi /\lambda$ is the light-wave number.

The Gaussian beam is a special solution of the Helmholtz equation under gradually varying amplitude approximation, which can describe the properties of laser beams well.96 The Helmholtz equation can then be solved for several structured laser beams based on the Gaussian beam. First and foremost, by solving the Helmholtz equation in the paraxial form, i.e., the paraxial wave equation, the well-known HG and LG modes can be solved in Cartesian coordinates and cylindrical coordinates, respectively, as shown in Figs. 3(a)–3(b).162^,163 The IG modes are also an important family of orthogonal solutions to the paraxial wave equation, which represents a continuous transition from LG to HG modes, as shown in Fig. 3(c).164^–166 Another set of solutions to the Helmholtz equation in free space, when solved in cylindrical coordinates, is the Bessel modes, as shown in Fig. 3(e).92^,167^,168 If solving the Helmholtz equation in elliptical cylindrical coordinates, Mathieu–Gauss beams can be obtained, as shown in Fig. 3(d).169^–171 Mathieu–Gauss beams are also one class of “nondiffracting” optical fields, which are a variant of the superposition of Bessel beams. Therefore, they have a similar capability of self-reconstruction after an opaque finite obstruction. Another important solution to the paraxial wave equation is the Airy beam, as shown in Fig. 3(f).172^,173 Similar to the Bessel modes, Airy beams exhibit unique properties of self-acceleration, nondiffraction, and self-reconstruction. Next, when solving the Helmholtz equation in parabolic coordinates, parabolic beams can be obtained, as shown in Fig. 3(g).160 Their transverse structures are described by parabolic cylinder functions, and contrary to Bessel or Mathieu beams, their eigenvalue spectra are continuous. Any nondiffracting beam can be constructed as a superposition of parabolic beams, since they form a complete orthogonal set of solutions of the Helmholtz equation. Based on parabolic beams, a new family of vector beams that exhibit novel properties is explored, i.e., parabolic-accelerating vector beams, as shown in Fig. 3(h).161 This set of beams obtains the ability to freely accelerate along parabolic trajectories. In addition, their transverse polarization distributions only contain polarization states oriented at exactly the same angle, but with different ellipticity. To sum up, the above-solved patterns we introduced are the eigenmodes of Helmholtz equations, with some examples shown in Fig. 3.

For eigenmode superposition theory, it was found that the LG mode can be generated by coherent superposition of the HG modes as early as 1992,90 as shown in Fig. 4(a). It can be conveniently understood by illustrating the above basic modes on a Bloch sphere, analogous to the Poincaré sphere (PS) for polarization, but for spatial modes. For example, if such a Bloch sphere is constructed with the ${\mathrm{LG}}_p$ modes, such as ${\mathrm{LG}}_{\mathrm{0,1}}$ and ${\mathrm{LG}}_{0,-1}$ on the poles, then the equator will represent superpositions of such beams: the HG modes.179 Due to the fact that these set of modes form an infinite basis, it allows one set of modes to be represented in terms of the other. Using relations between Hermite and Laguerre polynomials,90^,180$$\sum _{k=0}^{m+n}(2i{)}^k{P}_k^{(n-k,m-k)}(0)H_{n+m-k}(x)H_k(y)=2^{m+n}\times \{\begin{array}{cc}(-1{)}^{m}m!(x+iy{)}^{n-m}{L}_m^{n-m}(x^2+y^2)& \text{for}n\ge m\\ (-1{)}^{n}n!(x-iy{)}^{m-n}{L}_m^{m-n}(x^2+y^2)& \text{for}m>n\end{array},$$(5)$$P_k^{(n-k,m-k)}(0)=\frac{{(-1)}^k}{2^{k}k!}\frac{d^k}{d{t}^k}[(1-t{)}^n(1+t{)}^m]{|}_{t=0},$$(6)where $H_k(·)$ and $L_m^{n-m}(·)$ are Hermite and Laguerre polynomials, respectively, then LG modes could be represented in terms of superpositions of HG modes as181$${\mathrm{LG}}_{p,\pm l}(x,y,z)=\sum _{K=0}^{m+n}(\pm i{)}^{K}b(n,m,K)·{\mathrm{HG}}_{m+n-K,K}(x,y,z),$$(7)$$b(n.m,K)={\left[\frac{(N-K)!K!}{2^{N}n!m!}\right]}^{1/2}\frac{1}{K!}\frac{{\mathrm{d}}^K}{\mathrm{d}{t}^K}[(1-t{)}^n(1+t{)}^m]{|}_{t=0},$$(8)where $l=m-n$, $p=\min (m,n)$, and $N=m+n$. This leads to an alternative description of light fields through the perspective of mode superposition, particularly useful in the description of beams with a transverse profile that is invariant during propagation. For the mutual superposition and conversion of HG and LG eigenmodes, Abramochkin and Volostnikov in 2004 introduced a parameter $\alpha$ to unify them.182 Such beams with more universality are called generalized Gaussian beams or Hermite–Laguerre–Gaussian (HLG) beams. 41^,175^,182^,183 The expression of HLG beam is as follows: $$\begin{gathered} {\mathrm{HLG}}_{n,m}(\mathbf{r},\mathrm{z}|\alpha )=\frac{1}{\sqrt{2^{N-1}n!m!}}\exp (-\pi \frac{|\mathbf{r}{|}^2}{w}\left){\mathrm{HL}}_{n,m}\right(\frac{\mathbf{r}}{\sqrt{\pi }w}|\alpha ) \\ \times \exp [ikz+ik\frac{{\mathbf{r}}^2}{2R}-i(m+n+1)\mathrm{\Psi }(z)], \end{gathered}$$(9)where ${\mathrm{HL}}_{n,m}(•)$ are Hermite–Laguerre (HL) polynomials, $\mathbf{r}=(x,y{)}^{\mathrm{T}}={(r\cos \varphi ,r\sin \varphi )}^{\mathrm{T}}$, $R(z)=(z_R^2+z^2)/z$, $k{w}^2(z)=2(z_R^2+z^2)/z_R$, $\mathrm{\Psi }(z)=\arctan (z/z_R)$, and $z_R$ is the Rayleigh range. It was found that when $\alpha =0$ or $\pi /2$, the mode ${\mathrm{HLG}}_{n,m}$ will be reduced to ${\mathrm{HG}}_{n,m}$ or ${\mathrm{HG}}_{m,n}$ mode. When $\alpha =\pi /4$ or $3\pi /4$, the mode ${\mathrm{HLG}}_{n,m}$ will be reduced to ${\mathrm{LG}}_{p,\mp l}$ mode $[p-\min (m,n),l=m-n)]$. For other $\alpha$, the mode ${\mathrm{HLG}}_{n,m}$ is displayed as the beam distribution of multi-phase singularities. Take ${\mathrm{HLG}}_{\mathrm{3,1}}$ mode as an example, when $\alpha =0$, $\pi /4$, and $\pi /8$, the mode ${\mathrm{HLG}}_{\mathrm{3,1}}$ could be reduced to ${\mathrm{HG}}_{31}$, ${\mathrm{LG}}_{12}$, and mode with multi-phase singularities, as shown in Fig. 4(c).175 Since HLG modes are able to unify HG modes and LG modes, it was mapped in the PS to show the relationship among HLG, HG, and LG modes.174 As shown in Fig. 4(b), the poles represent the high-order LG modes with opposite topological charges, and the equator represents the high-order HG modes, while the mode between the poles and the equator represents the transitional high-order HLG modes.

On the basis of HLG modes, analyzing its coherent superposition can obtain a high-dimensional complex light field in a coherent state, whose typical type is SU(2) mode. The SU(2) mode appears when the laser mode undergoes frequency degeneracy with a photon performing as an SU(2) quantum coherent state coupled with a classical periodic trajectory,174^,177^,184^,185 which contains both spatially coherent wave packets and geometric ray trajectories, as shown in Fig. 4(e). Taking the HLG mode as the basic mode of SU(2) coherent state, the superposed SU(2) mode is expressed as174$$|{\psi }_{n,m.l}^{N,P,Q}⟩=\frac{1}{2^{N/2}}\sum _{K=0}^N{e}^{iK\varphi }{\left(\begin{array}{c}N\\ K\end{array}\right)}^{\frac{1}{2}}|{\psi }_{n+QK,m,l-PK}⟩,$$(10)where $\varphi$ is the phase term, and $P/Q$ ($P$ and $Q$ are coprime integers) is the ratio of the distance between the transverse mode and longitudinal mode leading to frequency degeneracy, i.e., the transverse mode and longitudinal mode of various eigenmodes should meet the coherent superposition condition.

Another similar superposition of the IG modes can form patterns with multi-singularity, named the helical IG (HIG) modes.186^–188 HIG modes are obtained by coherent superposition of even and odd IG modes, whose expression is $${\mathrm{HIG}}_{p,m}^{\pm }={\mathrm{IG}}_{p,m}^e(\xi ,\eta ,\epsilon )\pm i{\mathrm{IG}}_{p,m}^o(\xi ,\eta ,\epsilon ),$$(11)where $\pm$ is the direction of the vortex; $p$ and $m$ are the orders of the IG mode; $o$ and $e$ represent the odd mode and the even mode, respectively; $\epsilon$ is the ellipticity parameter, indicating the change degree of ellipticity. $\xi$ and $\eta$ are elliptic coordinates; and ${\mathrm{IG}}_{p,m}^{e,o}(·)$ represent the expression of IG modes.165 When $\epsilon \to 0$, ${\mathrm{IG}}_{p,m}^{e,o}$ modes could be reduced to ${\mathrm{LG}}_{p.l}$ modes with $l=m$ and $p=2n+l$. When $\epsilon \to \infty$, ${\mathrm{IG}}_{p,m}^{e,o}$ modes could be reduced to ${\mathrm{HG}}_{n_x.n_y}$ modes with $n_x=m-1$ and $n_y=p-m+1$. Therefore, for $\epsilon =0\to \infty$, the HIG modes composed of even and odd modes show specific distribution changes, shown in Fig. 4(d).176

Comparing HLG and HIG modes, it could be found that they all possess phase singularities with corresponding spatial distributions for differently composed HG and LG modes. The above HG, LG, HLG, and HIG modes belong to the general family of structured Gaussian modes, also known as the singularities hybrid evolution nature (SHEN) modes.178 The model expression of SHEN modes is $$\begin{gathered} {\mathrm{SHEN}}_{n,m}(x,y,z|\beta ,\gamma )=\sum _{K=0}^N{e}^{i\beta K}b(n,m,K), \\ •\{\begin{array}{cc}(-i{)}^K{\mathrm{IG}}_{N,N-K}^e(x,y,z|\epsilon =2/{\tan }^2\gamma ,& \text{for}(-1{)}^K=1\\ (-i{)}^K{\mathrm{IG}}_{N,N-K+1}^o(x,y,z|\epsilon =2/{\tan }^2\gamma ,& \text{for}(-1{)}^K\ne 1\end{array}. \end{gathered}$$(12)

When $\beta =\pm \pi /2$, SHEN modes could be reduced to HIG modes. When $\gamma =0$, SHEN modes could be reduced to HLG modes. When $(\beta ,\gamma )=(\mathrm{0,0})$ or $(\pi ,0)$, SHEN modes could be reduced to HG modes. When $(\beta ,\gamma )=(\pm \pi /\mathrm{2,0})$, SHEN modes could be reduced to LG modes. Therefore, SHEN modes can uniformly describe HG, LG, HIG, and HLG modes. In addition, the PS could be applied to define the SHEN sphere to describe these modes, as shown in Fig. 4(f).178

It can be seen that the above patterns are derived from the direct coherent superposition of the basic modes. The beam generated after superposition can be regarded as a new kind of eigenmodes with single-frequency operation. If performing coherent superposition between these eigenmodes, diverse and complex structured laser beam patterns could be generated. Moreover, in a practical resonator, if multiple modes interact coherently, the coupling of frequency and phase will be formed spontaneously to achieve TML. The principle of the TML effect97^–101 includes frequency locking and phase locking. The total electric field of a beam in the coherent superposition state can be given as99$$E_{\text{tot}}=\sum _{m,n}{a}_{m,n}X{G}_{m,n}(·)*\exp [i{\varphi }_{m,n}+ikz+ik\frac{x^2+y^2}{R(z)}-iq\psi (z)],$$(13)where $XG$ represents the polynomial of eigenmodes, such as HG, LG, and IG. The subscripts $m$ and $n$ are the order indices of the corresponding basic modes, $a_{m,n}$ is the weight of each basic mode, $\exp (\dots )$ is the phase item, ${\varphi }_{m,n}$ is the initial phase, and $q\psi (z)$ is the Gouy phase.

The spatial pattern is analyzed by superimposing the electric field of multiple modes with the locking phase, including the Gouy phase.189 Moreover, with the assistance of the inherent nonlinearity of the laser cavity, the frequencies of the composed modes are possible to be pulled to the same value,87^–89 and then the total electric field can be expressed as $$E_{\mathrm{tot}}(x,y,z)=\exp [i\frac{\overline{\omega }}{c}z+i\frac{\overline{\omega }}{c}\frac{x^2+y^2}{\overline{R(z)}}-i\overline{q}\psi (z)]·\sum _{m,n}{a}_{m,n}X{G}_{m,n}(·)*\exp (i{\varphi }_{m,n}),$$(14)where $\overline{\omega }$ is the averaged optical frequency, whose derivation is as follows: $$\{\begin{array}{l}\overline{\omega }={\omega }_0+\frac{\sum _{m,n}{a}_{m,n}\mathrm{\Delta }{\omega }_n}{\sum _{m,n}{a}_{m,n}}\\ \mathrm{\Delta }{\omega }_n={\omega }_n-{\omega }_0=\frac{c(k_x^2+k_y^2)}{2k_z}\end{array}.$$(15)

Here, ${\omega }_0$ is the optical frequency of the fundamental transverse mode, $\mathrm{\Delta }{\omega }_n$ is the frequency spacing between the $n$th mode and the fundamental mode, $c$ is the velocity of light, $k_x=\pi n/l_x$, $k_y=\pi n/l_x$, $k_z=2\pi /\lambda$, and $l_x$ and $l_y$ are the sizes of the cavity in the $x$ and $y$ directions, respectively. Along with the locking of frequencies, the parameters of $R(z)$ and index of $\psi (z)$ should also be an averaged one to help with the locking of the total phases. The cooperatively frequency-locked multimode regime, in which at least two transverse modes contribute significantly to the output field, and lock to a common frequency with which they oscillate in a synchronized way. The locking concerns also the relative phases of the modes, so that the output intensity has a stationary transverse configuration. The common oscillation frequency, cooperatively selected by the modes, corresponds to the average of the modal frequencies, weighted over the intensity distribution of the modes in the stationary state.

The patterns formed by TML effect could possess phase singularities in dark points.102 Around each of these phase singularities, the modulus of the electric field raises from zero in the form of an inverted cone with a steep gradient. If performing a closed counterclockwise loop that surrounds one of these points, the phase of the envelope of the electric field changes by a value equal to $\pm 2\pi m$, where $m$ is a positive integer. These properties are fulfilled also in the “optical vortices” discovered by Coullet and collaborators63 in their 2D analysis of the model.62 A major difference is that from the fact that the vortices in Ref. 63 can be generated in any position of the transverse plane, whereas the singularities that appear in the stationary configurations of a laser system are located in precisely defined positions, i.e., the dark points.

The stable beam pattern formed by coherent superposition through TML usually needs to meet the following conditions: First, there should be a large value of the Fresnel number to sustain such multi-transverse modes.85 Second, the transverse mode spacing, $\mathrm{\Delta }{v}_T$, should be small (several gigahertz or lower) to assist nonlinear coupling in the spectral band.190 Third, the interval between two neighboring vortices should also be small (usually tens of micrometers) for the formation of stable patterns.191 Fourth, a wide cavity without mechanical boundaries is also needed.87 The patterns produced by the eigenmode coherent superposition in the TML state include optical lattice (OL) and OVL,86^,88^,89 which could be obtained in vertical-cavity surface-emitting lasers (VCSELs)87 and solid-state lasers,88^,89^,99^,192 as shown in Figs. 5(a)–5(e). In addition to coherent superposition, incoherent superposition can also produce patterns similar to OL,193^,195 as shown in Figs. 4(f) and 4(g). The incoherent superposition is to analyze the output OL pattern through the superposition of intensities of the composed modes alone. It is pointed out that in multi-transverse-mode lasers, the coupling between transverse modes occurs through their intensities rather than their field amplitudes, and these modes are arranged according to the principle of transverse hole burning to maximize energy coexistence and minimize intensity distribution overlap. It is found that the beam patterns generated by incoherent superposition have higher symmetry, and there may be no phase singularity in some dark areas of the pattern.194

We have summarized the principle of directly generating spatially structured beams from the laser cavity, namely, the eigenmode superposition theory. The spatial characteristics of the spontaneous organized patterns are explained by the interaction and superposition of the oscillation modes. However, with the help of some modulation devices, such as the spiral phase plate,196^–198 diaphragm,199 acousto-optic modulator,200 liquid crystal Q-plate,201^–205 J-plate,145 liquid crystal SLM,206^–208 and digital micromirror device,209^–211 various spatial structure laser beams can also be generated indirectly. There are also many reviews40^,42^,43^,45^–47^,50^,212 on this part of active regulation to generate spatially structured laser beams, and more detailed information can be found in those reviews.

As for the study of structured laser pattern formation, the traditional electromagnetic field equations including MB and Helmholtz equations were adopted in recognition of the importance of gain and loss. In addition, the eigenmode superposition theory makes it possible to form diverse and complex beam patterns. When the laser oscillates simultaneously in multiple modes and the phase difference between them is stable, the mode locking occurs. What we talked about the spatial characteristics of laser transverse modes in Sec. 3 is to study the TML under the condition of single longitudinal mode. However, if multiple longitudinal modes are involved, total mode locking or spatiotemporal locking will occur,103^–106 thus generating spatiotemporal laser beams.

The spatiotemporal mode locking is often realized by fiber lasers, referring to the coherent superposition of longitudinal and transverse modes of the laser, which allows locking multiple transverse and longitudinal modes to create ultrashort pulses with various spatiotemporal distributions, as shown in Figs. 6(a1) and 6(a2). The locking of transverse and longitudinal modes of a laser is realized by spatial filtering107 and spatiotemporal normal dispersion mode locking,116^,117 respectively. The spatiotemporal mode locking can be realized through the high nonlinearity, gain, and spatiotemporal dispersion of the optical fiber medium, as well as spectral and spatial filtering.103 These inseparable coupling effects can be described by the cavity operator $\hat{C}$ as follows:107$$\widehat{C}=\widehat{F}(x,y)\widehat{F}(\omega )\widehat{SA}(x,y,t)\widehat{P}(x,y,t),$$(16)where $\hat{F}(x,y)$ and $\hat{F}(\omega )$ are the spectral and spatial filter functions, respectively, $\widehat{SA}(x,y,t)$ is the spatiotemporal saturable absorber transfer function, and $\hat{P}(x,y,t)$ accounts for the effect of the pulse propagation through the three-dimensional (3D) nonlinear gain medium. $\hat{P}$ includes the inseparable effects of 3D gain, such as spatiotemporal dispersion and nonlinear mode coupling. With the composition of iterated nonlinear projection operations, the field of spatiotemporal locking pulse can be expressed as $$E_{i+1}(x,y,t)=\widehat{C}{E}_i(x,y,t),$$(17)where the subscript of $E$ is the round-trip number. In each round trip, the nonlinear dissipation of $\hat{C}$ is selected from the field certain attributes, and the saturable laser gain provides a conditional (frequency and energy-limited, and spatially localized) rescaling of the selected field.

The schematic diagram of the cavity supporting spatiotemporal mode locking is shown in Fig. 6(a3). The fiber ring laser was composed by offset splicing a graded-index fiber to a few-mode (three modes were supported) Yb-doped fiber amplifier, which leads to spatial filtering action.107 Spatial filtering can lock multiple transverse modes by controlling the overlap of fields coupled to the optical fiber. Then, the self-starting mode locking in the normal chromatic dispersion regime is achieved using a combination of spectral filtering and intracavity nonlinear polarization rotation, which is realized in the longitudinal mode locking. Through the space–time locking of the transverse and longitudinal modes, ultrashort pulses with special space–time distribution can be obtained. In the process of spatiotemporal mode locking, the mode dispersion will affect the locking effect, and the small mode dispersion of graded-index multimode fiber is considered to be a key factor to make spatiotemporal mode locking possible.103 Experimental regimes of spatiotemporal mode locking and results from a reduced laser model are shown in Fig. 6(b).107 The reduced models predicted how the effects of disorder, and the increased dimension of the optimization, affect the regimes of spatiotemporal mode locking. On this basis, it was found that spatiotemporal mode locking can also be realized in multimode fiber lasers with large mode dispersion, in which the intracavity saturable absorber plays an important role in offsetting the large mode dispersion.110 Spatiotemporal mode locking at a fiber laser using a step-index few-mode thulium fiber amplifier and a semiconductor saturable absorber was also reported.113 The former realizes spatial filtering to lock the transverse mode, and the latter plays a role in longitudinal mode locking.

Therefore, spatiotemporal mode locking is affected by gain, spatial filtering, optical nonlinear interaction between saturable absorbers, and optical fiber medium, as well as the coupling between temporal and spatial degrees of freedom.107 Apart from multimode fiber lasers, in all few-mode fiber, it is realizable to obtain spatiotemporal mode locking to create bound-state solitons.109 In addition, the scanning output beam can be generated by spatiotemporal locking of the laser mode,114 as shown in Fig. 6(c). The phase locking of the longitudinal and transverse (${\mathrm{TEM}}_{00}$ and ${\mathrm{TEM}}_{01}$) modes is simply obtained by tilting the pump laser end mirror to induce time-varying pulse coupling in a photonic crystal fiber for subsequent generation of frequency-shifted Raman solitons. The introduced spatial oscillations of the output beam lead to modulation of the coupling efficiency of the fiber and effectively induces wavelength sweeping.

The spatiotemporal mode-locked pulses directly produced by fiber lasers are often irregularly distributed. Another method to generate spatiotemporal beams with regular and complex distribution is to use the pulse-shaping device based on SLM. The designed pulse shaper is usually applied to shape the input femtosecond laser to obtain the specific spatiotemporal pattern. As shown in Fig. 7(a), the spatiotemporal optical vortices have been proved to be generated using spiral phase in the pulse shaper.118 Suppose an optical field in the spatial frequency–frequency domain ($k_x-\omega$) is given by $g_R(r)$. After a spiral phase of $e^{-il\theta }$ is applied, a 2D Fourier transform gives the field in the spatial-temporal $(x,t)$ domain as follows: $$G(\rho ,\varphi )=\mathrm{FT}\{g_R(r){\mathrm{e}}^{-il\theta }\}=2\pi (-i{)}^l{\mathrm{e}}^{-il\theta }{H}_l\{g_R(r)\},$$(18)where $(r,\theta )$ are the polar coordinates with $r=\sqrt{k_x^2+{\omega }^2}$ and $\theta ={\tan }^{-1}(\omega /k_x)$, and $(\rho ,\varphi )$ are the Fourier conjugate polar coordinates with $\rho =\sqrt{x^2+t^2}$ and $\theta ={\tan }^{-1}(x/t)$. Here, $H_{\mathrm{l}}\{g_R(r)\}={\int }_0^{\infty }{rg}_R(r)J_{\mathrm{l}}(2\pi \rho r)\mathrm{d}r$ and $J_l$ is the Bessel function of the first kind.

Therefore, starting from chirped mode-locked pulses, a diffraction grating and cylindrical lens disperse frequencies spatially and act as a time-frequency Fourier transform. Then, a spiral phase on the SLM and an inverse Fourier transform by recollecting dispersed frequencies with a grating-cylindrical lens pair form the chirped spatiotemporal vortex. The full electric field is presented as $$E(\rho ,\varphi )=G(\rho ,\varphi )\exp (i{k}_{z}z-i\omega t).$$(19)

After generating the spatiotemporal vortex pulse, it travels through an afocal cylindrical beam expander and stretches in the direction of the vortex line. It is reported that the stretched spatiotemporal vortex pulse could transform into a toroidal vortex pulse through a conformal mapping system formed by two SLMs,126 as shown in Fig. 7(b). In addition, the spatiotemporal optical vortex was also demonstrated to be generated from a light source with partial temporal coherence and fluctuating temporal structures.119 Similarly, through a phase mask in SLM, interesting wave packets, such as diffraction-free pulsed beams with arbitrary 1D transverse profiles without suffering power loss were generated.121 The basic concept [illustrated in Fig. 7(c)] combines spatial-beam modulation and ultrafast pulse shaping and is related to the so-called $4f$-imager used to introduce spatiotemporal coupling into ultrafast pulsed beams. The modulated beam is reflected back, and the pulse is reconstituted by the grating to produce the spatiotemporal light sheet. Additionally, it applied reflective annular mask in a pulse shaper to generate a spatiotemporal Bessel wave packet,122 as shown in Fig. 7(d). Since the mask has an annular shape, it is then possible to obtain a spatiotemporal Bessel beam at its waist by doing the inverse Fourier transform in the space and time domains of the signal reflected by the mask. This analysis has revealed that these beams are produced by a superposition of plane waves of different optical frequencies and directions of propagation traveling at the same group velocity along the $z$ axis. With all plane waves added in the same phase, a nondiffraction spatiotemporal beam can be generated through spatiotemporal coupling.124

In addition, a device for generating an arbitrary vector spatiotemporal light field with arbitrary amplitude, phase, and polarization at each point in space and time was designed.125 As shown in Fig. 7(e), the laser output with two orthogonal polarizations propagates through the pulse shaper to redistribute between the space domain and the time domain. The shaped light propagates through the multi-plane light conversion (MPLC) device and is converted to different HG modes at the output port of the MPLC. Then, arbitrary spatiotemporal beams can be generated through the design and combination of HG beams at different times. These methods of transforming spatiotemporal beams through optical devices, such as pulse shapers, gratings, and lenses can effectively generate spatiotemporal beams with specific structures. They can be used in the fields of imaging, optical communication, nonlinear optics, particle manipulation, and so on.

For the booming research on the spatial and spatiotemporal properties of structured laser beams reviewed in the above sections, investigations are based on beams at a single wavelength. Currently, the nonlinear transformation technology for fundamental mode Gaussian beams is very mature. The combination between structured laser beams and nonlinear transformation on the transverse pattern variation has been of great interest in recent years. The SFG,127^–130 SHG,131^–140 FWM,141^,142 and other frequency upconversion143^–145 methods have been studied in the nonlinear process of structured laser beams. The variation of OAM in the nonlinear process are one of the focuses of these studies. In this section, the nonlinear process of structured laser beams is introduced from two aspects: external-cavity modulations and intracavity transformation. We will first present the physical mechanisms.

Generally, the nonlinear transformation of structured patterns is based on the nonlinear wave equation, $$\frac{\partial E}{\partial z}=\frac{i\omega }{2{\epsilon }_{0}cn}{P}^{\mathrm{NL}}{e}^{i\mathrm{\Delta }kz},$$(20)where $E$ is the electric field, $\omega$ is the optical frequency, $P^{\mathrm{NL}}$ is the nonlinear polarization, and $\mathrm{\Delta }k$ is the wave vector difference between the polarized wave and the incident light. The nonlinear process in the multi-wave mixing process can be obtained by solving the coupled wave equations. Generally speaking, for the $n$’th-order nonlinear effect, $n+1$ nonlinear coupled wave equations corresponding to different frequencies can be listed. By simultaneously solving the $n+1$ coupled wave equations, the electric field strengths of these different frequencies of light can be obtained, thereby leading to the law of mutual conversion of energy between these light fields. In the nonlinear transformation of structured patterns, the second-order nonlinear effect is the main part, including SFG and SHG. Consider three monochromatic plane waves $E_1$, $E_2$, and $E_3$ propagating in the $z$ direction with frequencies ${\omega }_1$, ${\omega }_2$, and ${\omega }_3$, respectively. Considering only the second-order nonlinear effect, the second-order nonlinear polarization can be written as $$\{\begin{array}{l}{P}^{(2)}({\omega }_1)=2{\epsilon }_0{\chi }^{(2)}(-{\omega }_1;{\omega }_3,-{\omega }_2)·E_3{E}_2^{*}\\ P^{(2)}({\omega }_2)=2{\epsilon }_0{\chi }^{(2)}(-{\omega }_2;{\omega }_3,-{\omega }_1)·E_3{E}_1^{*}\\ P^{(2)}({\omega }_3)=2{\epsilon }_0{\chi }^{(2)}(-{\omega }_3;{\omega }_1,{\omega }_2)·E_1{E}_2\end{array},$$(21)and we can get the coupled wave equations for three-wave interaction as $$\{\begin{array}{l}\frac{d{E}_1(z)}{dz}=\frac{i{\omega }_1}{c{n}_1}{\chi }^{(2)}(-{\omega }_1;{\omega }_3,-{\omega }_2)·E_3(z)E_2^{*}(z)e^{i\mathrm{\Delta }kz}\\ \frac{d{E}_2(z)}{dz}=\frac{i{\omega }_2}{c{n}_2}{\chi }^{(2)}(-{\omega }_2;{\omega }_3,-{\omega }_1)·E_3(z)E_1^{*}(z)e^{i\mathrm{\Delta }kz}\\ \frac{d{E}_3(z)}{dz}=\frac{i{\omega }_3}{c{n}_3}{\chi }^{(2)}(-{\omega }_3;{\omega }_1,{\omega }_2)·E_1(z)E_2(z)e^{i\mathrm{\Delta }kz}\end{array}.$$(22)

Then, the field intensity of a specifically structured light beam after nonlinear transformation can be obtained by substituting the structured light field expression XG (e.g., HG, LG, and IG) into the coupled wave Eq. (22) and solving them.

External cavity pattern modulations and nonlinear interactions are the main form of nonlinear transformation in structured laser beams. The first research on the transformation of structured laser beams in nonlinear optics began with the SHG of LG modes in 1996.131 It was found that the SHG fields carry twice the azimuthal indices of the pump, which provided straightforward insight into OAM conservation during nonlinear interactions at the photon level. The relationship among the OAMs of the input $l_1,l_2,\dots$ and output beams $l$ was recognized to follow the law of $l=l_1+l_2+\dots +l_n$. That is, OAM is conserved in the nonlinear process. As such, for SHG modes of two photons with angular frequency $\omega$ and a single OAM, if the OAMs are equal, it has $l_{2\omega }={2l}_{\omega }$ or $l_{2\omega }=l_{{\omega }^{\prime }}+l_{{\omega }^{″}}$,135 as shown in Fig. 8(a). This conservation law is also applicable to fractional and odd-order OAM beams.134 The generation of LG beams with higher radial orders and IG beams through a nonlinear wave mixing process was further investigated to obtain more complex beam patterns.130^,139^,140 However, in the above studies, the characteristics of the frequency-doubled beam patterns during propagation have hardly been mentioned. Later, in the research of SHG modes through input LG beams with opposite OAMs, the near- and far-field patterns show different light field distributions,137 as shown in Fig. 8(b). In addition, for the change of pattern transmission, a more detailed theoretical model is proposed to describe the beam pattern transmission and radial mode transition in the process of SHG, and the results agree well with the simulations,145 as shown in Fig. 8(c). Apart from the single OAM state, phase structure transfer in FWM142 and sum frequency129 processes were also investigated for the input beams possessing coherent superposition of LG beams.

As shown in Fig. 8(d), there are two sets of patterns and propagation behaviors: (1) one pump beam carries OAM superposition mode with another pump beam carrying a single OAM mode and (2) both pump beams carry OAM superposition modes. The relationship between the SFG beam and the pump beam is as follows:129$$E_{\mathrm{SFG}}\propto \{\begin{array}{l}(L{G}_0^l+e^{i\theta }L{G}_0^{-l})*L{G}_0^l\to L{G}_0^{2l}+e^{i\theta }L{G}_l^0\\ (L{G}_0^{l_1}+e^{i\theta }L{G}_0^{-l_2})*L{G}_0^{l_2}\to L{G}_0^{l_1+l_2}+e^{i\theta }L{G}_{l_2}^0\\ (L{G}_0^l+e^{i{\theta }_1}L{G}_0^{-l})*(L{G}_0^l+e^{i{\theta }_2}L{G}_0^{-l})\to L{G}_0^{2l}+e^{i({\theta }_1+{\theta }_2)}L{G}_0^{-2l}+(e^{i{\theta }_1}+e^{i{\theta }_2})L{G}_l^{*0}\end{array},$$(23)where $L{G}_0^l$ represents the standard LG mode, and $\theta$ is the phase item. It is worth noting that $L{G}_l^{*0}$ is similar to the standard LG mode $L{G}_l^0$, but differs by a factor of 2 in the Laguerre polynomials. This difference makes the intensity in the radial direction of the SFG beam decrease much more rapidly than the standard LG mode.

All these above studies on nonlinear processes were explored on the basis of external cavity structured laser pattern generation. Usually, in these studies, structured beams were first generated with the help of modulation devices (such as SLM), and then frequency conversion was carried out. For patterns generated through intracavity nonlinear process, some studies showed new properties. In Fig. 9(a1), it shows a frequency-doubled cavity that converts the infrared fundamental frequency of Nd:YAG ($\lambda =1064\mathrm{nm}$) to the second-harmonic green ($\lambda =532\mathrm{nm}$) through an intracavity nonlinear crystal (KTP).146 The concept of the laser design exploits a unique feature of OAM coupling to linear polarization states. The resonant mode morphs from a linearly polarized Gaussian-like enveloped beam at one end of the cavity to an arbitrary angular momentum state at the other. A polarizer was required for selection of the horizontal polarization state before the J-plate, and the polarization of the light traversing the J-plate was controlled by simply rotating the J-plate itself. Various measured states from the laser, displayed on a generalized OAM sphere are shown in Fig. 9(a2). The transition patterns from one to the other allow visualization of lasing across vastly differing OAM values as superpositions with two concentric rings. Then, in a digital laser for on-demand intracavity selective excitation of second-harmonic higher-order modes, an SLM used for structured beam generation also acted as an end mirror of the laser resonator,147 as shown in Fig. 9(b1). After SHG modes passed through the nonlinear KTP crystal, it was found that the near-field spatial intensity profiles of the SHG LG modes in Fig. 9(b3) are similar to the intensity profile of the fundamental LG pump modes in Fig. 9(b2). But at the far field, the spatial intensity profiles of the SHG LG modes in Fig. 9(b4) are different from the fundamental pump modes because there is an added central intensity maximum, while in another intracavity SHG generation laser, the spatial distributions of the SHG beams are almost the same as that of the pump beams,148 as shown in Figs. 9(c2)–9(c3). For some SHG patterns, the topological charge was found to have doubled, as shown in Fig. 9(c4). The generation of high-order modes was obtained by the off-axis displacement of the output coupling mirror and the SHG process was through the intracavity BBO crystal, as shown in Fig. 9(c1). In addition, investigations on the SHG structured laser beams in the TML states have been carried out.149 Through a sandwich-like microchip laser composed of Nd:YAG, Cr:YAG, and LTO crystals in Fig. 9(d1), complex and diverse structured beams in TML states and their SHG beams were generated by altering the pumping parameters. As shown in Figs. 9(d2)–9(d3), a set of TML beams composed of the HG and LG modes and their SHG beams were obtained experimentally and agreed well with the theoretical simulation model as follows: $$\begin{gathered} E_{\mathrm{SHG}}(r,\phi )\propto [X{G}_{m1,n1}(r,\phi )+e^{i\varphi }X{G}_{m2,n2}(r,\phi )]\times [X{G}_{m1,n1}(r,\phi )+e^{i\varphi }X{G}_{m2,n2}(r,\phi )] \\ =X{G}_{m1,n1}^2(r,\phi )+2e^{i\varphi }X{G}_{m1,n1}(r,\phi )X{G}_{m2,n2}(r,\phi )+e^{i2\varphi }X{G}_{m2,n2}^2(r,\phi ). \end{gathered}$$(24)

The complex transverse patterns in the TML states were composed of different basic modes with different weight coefficients and different locking phases, which makes the spatial information of the fundamental frequency mode and its SHG beam quite abundant.

In summary, combining the nonlinear transformation with the study of structured laser beams, the beam patterns are endowed with richer spatial information characteristics. For external cavity nonlinear process of structured laser beams, the law of OAM conservation during nonlinear interactions of LG beams was found. For SHG and SFG modes of the special LG beams, the propagation of the output beam patterns from near-field to far-field shows varying spatial characteristics. For intracavity nonlinear processes of structured laser beams, much more complex and diverse beam patterns could be obtained. In general, as a new research field of structured laser beams, the nonlinear process of beam shaping can be widely used in 3D printing, optical trapping, and free-space optical communication. In addition, as reviewed in Secs. 3 and 4, since there are many techniques for generating spatial and spatiotemporal structured beams. By applying nonlinear transformation technology, it is expected that the future of structured laser beams will have broader development prospects.

This paper is dedicated to reviewing the evolution of the spatial patterns of structured laser beams, covering the spontaneous organization of patterns described by relative equations and the advancements of on-demand transformations of laser patterns. Taking the spatial pattern as the core, we first reviewed the theoretical basis of laser transverse mode formation and emphasized its electromagnetic field properties and the dynamic mechanisms described by the related equations. Then, we analyzed the latest developments in the spatial characteristics of structured laser beam patterns through eigenmode superposition theory. With the coherent and incoherent superposition of laser eigenmodes, complex and diverse spatial patterns of structured laser beams can be generated. These studies on the spatial characteristics of structured laser beams are often conducted under the premise of a single longitudinal mode. However, if multiple longitudinal modes are involved, the time dimension needs to be accounted for. Therefore, we later reviewed the research on spatiotemporal structured laser beams, including direct generation by spatiotemporal mode-locking effect in fiber lasers and indirect regulation through the pulse shaper based on SLM. Moreover, it was found that the structured laser patterns could be endowed with richer spatial information characteristics through nonlinear conversion processes. We finally reviewed various nonlinear processes of structured laser patterns ranging from external cavity modulations to intracavity transformation comprehensively. Looking back over these 10 years, we can see how much our research and understanding of laser spatial features have advanced from classical to quantum,213 especially since the discovery of OAM in the 1990s. However, the study of structured laser beams may just be in its early stages. We still have many unexplored novel phenomena and theories. There is potential for new and improved applications based on these spatial and temporal properties of laser modes, which could facilitate further research on novel laser spatial structures.

Biographies of the authors are not available.