## Abstract

We introduce a simplified version of the steady-state *ab initio* laser theory for calculating the effects of mode competition in continuous wave lasers using the passive cavity resonances. This new theory harnesses widely available numerical methods that can efficiently calculate the passive cavity resonances, with negligible additional computational overhead. Using this theory, we demonstrate that the pump profile of the laser cavity can be optimized both for highly multi-mode and single-mode emission. An open source implementation of this method has been made available.

© 2016 Optical Society of America

## 1. Introduction

There has been great recent interest in using spatially nonuniform pumping of a laser to control the number and choice of lasing mode(s) [1–7]. While previous works have involved both empirical approaches and those guided by theory and simulations, the latter currently have drawbacks which limit their convenience and applicability to detailed optimization studies. Historically, the design and optimization of a laser begins and ends with design of the laser cavity. This approach has been used out of both convenience and necessity; many simulation tools can easily calculate the eigenmodes of a passive cavity, but it is difficult to generalize these tools to include the effects of the gain medium, such as mode competition, gain saturation and spatial hole-burning. For example, auxiliary equations can be added to the finite difference time domain (FDTD) method to account for these effects, but these add significant computational overhead [8–12]. Frequency domain techniques, such as the steady-state *ab initio* laser theory (SALT), can provide an exact treatment of both the cavity geometry and gain medium, but no public implementation is available [13–15]. In lieu of a full treatment of the gain medium, the highest *Q* eigenmodes of the passive cavity are assumed to be the lasing modes, and in practice this ansatz works reasonably well provided that the cavity is uniformly pumped. However, lasing modes are a function of both the cavity geometry and the spatial gain distribution within the cavity, and the laser properties can be significantly altered in the presence of non-uniform pumping. Recent experimental and theoretical results have shown that optimizing the spatial pump profile can provide additional degrees of freedom, enabling the selection of individual lasing modes [1, 3, 4, 6], increasing the slope efficiency [5], adding functionality by enabling tunable behavior [2], or increasing significantly the number of lasing modes at a given pump value [7]. While these works illustrate the potential impact of using non-uniform pumping to optimize the laser behavior, optimizing the spatial pump distribution experimentally is time consuming and the performance gain can be difficult to predict beforehand.

In this work, we present an analytic method and associated simulation tool which enables non-uniform pumping to be incorporated into laser design from the outset. Specifically, we adapt an analytic approximation to SALT (SPA-SALT, the single pole approximation) [14] so that it can use the passive cavity resonances as an input. The passive cavity resonances can then be calculated using existing electromagnetic field simulation tools (e.g. FDTD, FEM), after which SPA-SALT solves for the lasing thresholds and modal intensities as a function of the spatial pump distribution while accurately accounting for the effects of mode competition, gain saturation and spatial hole-burning. This approach is valid when line pulling effects (including frequency locking [16]) are negligible, such as for most semiconductor microcavity lasers, as well as other laser systems with relatively high-Q passive cavities. It provides a computationally efficient method for including the effects of non-uniform pump distributions in laser design. To illustrate breadth of this technique, we use this algorithm to optimize the spatial pump profile in a multi-mode chaotic cavity laser to achieve either highly multi-mode lasing, or single mode lasing in the same cavity. Furthermore, we confirm the validity of this approximation through comparison with full SALT simulations. Finally, an open source implementation of this resonance SPA-SALT technique based on COMSOL is available in Code 1 (Ref. [17]).

The remainder of this paper is organized as follows, in Sec. 2 we provide the derivation of the resonance SPA-SALT equations. Section 3.1 shows semi-quantitative agreement between resonance SPA-SALT and exact simulations of the above threshold lasing behavior calculated using SALT, demonstrating that the passive cavity formulation of SPA-SALT is sufficient for guiding device design. Section 3.2 reports on enhancing the multi-mode behavior of cavities through numerical non-linear optimization of the non-uniform pump profile. In Sec. 3.3, we then show how changing the pump profile can be used to suppress multi-mode behavior, again finding semi-quantitative agreement between SPA-SALT and SALT, and demonstrating that single-mode behavior can be promoted through optimization of the pump profile. Finally, Sec. 4 will offer some concluding remarks.

## 2. Passive single pole approximation

As the SPA-SALT equations are based on SALT, which provides a quite general and accurate theory of multimode steady state lasing, it is useful to provide a brief overview of that theory. SALT was first derived nearly a decade ago as a frequency-domain formulation of the semi-classical Maxwell-Bloch equations in steady-state, which can be solved efficiently to provide a nearly exact description of the spatial degrees of freedom of the laser system [13–15]. SALT has two features that distinguish it from previous approaches to solving the Maxwell-Bloch equations, the ability to treat cavities with an arbitrary geometry, such as chaotic or random lasers [18–21], and the capability to describe essentially exactly the space-dependent saturation of the gain medium (spatial hole-burning). The fundamental SALT equations are coupled non-linear wave equations for each active lasing mode, which take the form:

*N*lasing modes interact through the non-linear space-dependent saturation of the gain medium, which for a two-level Bloch atomic system is written as

_{L}**Ψ**

*(*

_{μ}**x**) and

*ω*∈ ℝ are the spatial profile and frequency of the lasing modes,

_{μ}*c*is the speed of light in vacuum,

*ε*is the dielectric function of the passive cavity, which is contained in a spatial domain denoted by

_{c}*C*,

*n*

_{0}is the index of refraction outside the cavity,

*D*

_{0}(

**x**) is the pump strength,

*ω*is the atomic transition frequency,

_{a}*γ*

_{⊥}is the gain width (polarization dephasing rate), Γ

*is the Lorentzian gain factor ${\mathrm{\Gamma}}_{\nu}={\gamma}_{\perp}^{2}/\left({\left({\omega}_{\nu}-{\omega}_{a}\right)}^{2}+{\gamma}_{\perp}^{2}\right)$, and the pump strength and fields have been written in normalized units [13, 14]. As lasing modes are self-generated within the cavity, they must satisfy a purely radiating (Sommerfeld) boundary condition,*

_{ν}*r*≡ |

**x**|, and

*d*is the dimensionality of the system [22]. Enforcing this purely outgoing boundary condition upon Eq. (1) results in a quantization condition on the allowed frequencies of the lasing modes. Taken together, Eqs. (1)–(3), comprise the SALT equations,

*N*coupled differential equations, one for each active lasing mode, where

_{L}*N*is determined self-consistently as the pump strength,

_{L}*D*

_{0}, is varied. The SALT equations are usually solved by introducing a complete set of constant flux (CF) states at every outgoing frequency by making use of the quantization provided by the outgoing boundary condition [14], however direct solution methods are also possible [23]. The SPA-SALT equations used here are most easily derived from the CF-state formulation [14].

Unfortunately, the explicit numerical implementation of the outgoing boundary condition, Eq. (3), can be challenging, especially in multiple dimensions, as it is frequency dependent. Outgoing boundary conditions are usually implemented numerically in an implicit manner, without directly specifying the outgoing frequency, through the use of an impedance matched absorbing region surrounding the finite simulation domain [24]. This inability to specify an arbitrary outgoing frequency makes it difficult for these implicit methods to solve for the basis of CF states needed for the SPA-SALT approximation. Instead, without adding gain to the cavity, using such an implicit outgoing boundary condition naturally yields the passive cavity resonances (as a subset of all of the modes of the finite system); the resonances satisfy

*ω̃*∈ ℂ is the (complex) frequency of the passive cavity resonance, and

_{m}*ε*(

_{abs}**x**) is the impedance-matched absorbing boundary layer at the edges of the simulation domian. The pairs {

*ω̃*,

_{m}

*φ**} constitute a countably infinite set, quantized by the Dirichlet boundary condition at the edge of the finite simulation domain. The difference between the threshold lasing modes, which can each be expressed as a single CF state, and the passive cavity resonances is critical when considering line pulling effects from the gain medium, as the lasing frequency is not necessarily given by the real part of the passive cavity resonance. This distinction is especially pronounced in low-*

_{m}*Q*“bad cavity” systems such as random lasers, where the width of the gain curve can be much less than the decay rate of the cavity,

*γ*

_{⊥}≪

*γ*= −2Im[

_{c}*ω̃*] [25]. However, for most traditional laser systems,

_{m}*γ*≪

_{c}*γ*

_{⊥}, which results in negligible line-pulling effects, and thus the frequencies and spatial profiles inside the cavity of the passive cavity resonances and the relevant active cavity CF states are nearly identical [13].

The single pole approximation was derived as a simplified form of the SALT equations, and makes use of the fact that the non-interacting lasing modes at threshold are each given by exactly one CF state at the lasing frequency [13, 14]. Here, we exploit this similarity between the dominant CF state for each lasing mode and the passive cavity resonances to derive the SPA-SALT equations in terms of the passive cavity mode frequencies and spatial profiles, letting **Ψ*** _{μ}*(

**x**) =

*a*

_{μ}

*φ**(*

_{μ}**x**). The derivation of the resonance version of SPA-SALT is very similar to the derivations using CF-states [14], so we will only highlight the major differences here, and provide all of the equations necessary for numerical solution of the problem.

Assuming that we have used a separate numerical package such as COMSOL Multiphysics to solve for the frequencies and spatial profiles of the passive cavity resonances, we renormalize the modes over the volume of the cavity, rather than the entire simulation domain, as

The SPA-SALT approximation assumes the lasing modes and frequencies are known and need not be obtained self-consistently (in the resonance approximation they are determined by Eq. (4)). With this assumption Eqs. (1) can be inverted as in [14], to yield

in which ${D}_{0}^{(\mu )}$,*I*= |

_{μ}*a*|

_{μ}^{2}are respectively the non-interacting lasing threshold and intensity of the

*μ*th lasing mode, constrained to be positive. The modal overlap is given by

*χ*, and the effects of a spatially varying pump through its appearance in the non-interacting threshold equation, (6).

_{μν}Despite the relative simplicity of Eq. (8), it does not immediately specify the number of active lasing modes for any arbitrary pump value, and is instead dependent upon the non-interacting threshold pump values. The interacting threshold pump values are determined from their respective non-interacting values as,

in which*λ*∈ [0, 1] is the generalized mode competition parameter defined in [14],

_{μ}*λ*= 0, and the interacting thresholds are identical to their non-interacting counterparts, while

_{μ}*λ*= 1 indicates gain clamping, where the

_{μ}*μ*th mode never reaches threshold. Finally, after calculating the interacting mode thresholds using Eqs. (10) and (11), one can solve for the modal intensities of the lasing modes at any pump value as, Thus, using Eqs. (10) and (15), the above-threshold interacting semi-classical properties of lasers can be calculated from the knowledge of the passive cavity resonances with little additional computational effort.

Resonance SPA-SALT provides a convenient tool for studying any kind of cavity with a complex geometry for which the resonances can be efficiently calculated numerically, e.g. photonic crystal lasers or various kinds and shapes of microcavity lasers. Computationally, solving the resonance SPA-SALT equations requires solving the sparse eigenvalue problem given in Eq. (4) once for the passive cavity resonances, and then performing a few vector multiplication operations. In contrast, the most efficient SALT algorithms require first resolving a sparse eigenvalue problem for the lasing modes, before performing a similar number of vector multiplication steps for each value of the above threshold pump, *D*_{0} [23]. As such, when considering a uniform gain profile, the speedup provided by using resonance SPA-SALT is given by the number of above threshold pump values that one would need to solve for using SALT, which will usually yield at least an order of magnitude increase in performance. Once the resonances are known, the effect of the spatial distribution of the pump can be included with negligible computational effort through changing the parameter
$\overline{{f}_{\mu}}$ in Eq. (6). Optimization of specific laser properties via non-uniform pumping can then be modeled. In the next section we will apply this formalism to a specific case, the optimization of a chaotic cavity laser for highly multimode operation; to validate the method we will compare the results of resonance SPA-SALT with full SALT simulations.

## 3. Results

#### 3.1. Optimizing multimode behavior through passive cavity design

One way to design a low spatial coherence light source is to construct a laser with many independent lasing modes [26–28]. If the cavity is sufficiently complex, each lasing mode has a distinct spatial field pattern, and thus adding the emitted fields of many modes leads to a reduction in the spatial coherence. As an initial comparison of the passive cavity formulation of SPA-SALT with SALT, we choose to study chaotic “D-shaped” cavities which have recently been shown experimentally to generate laser emission with low spatial coherence [28]. D-shaped cavities consist of a disk with radius *R*, with a section removed along a chord parameterized by *r*_{0}, as shown in the inset of Fig. 1. These cavities are known to support chaotic ray dynamics [29,30], such that if one neglects the out-coupling losses and considers the system as an ‘ideal billiard,’ generic ray orbits for the D-shaped cavity cover ergodically the entire area of the cavity.

Broadly speaking, there are three requirements that must be satisfied in the design of a laser cavity suitable as an incoherent light source. First, there must be a large density of passive cavity modes with similar *Q*-factors close to the atomic resonance, such that the device has the potential for many lasing modes. Second, the lasing modes must have distinct transverse fields patterns so that the total field tend to self-average (longitudinal modes of a linear cavity do not have this property). Third, the mode-competition between these modes needs to be minimized, so that all of these modes are able to reach threshold even in the presence of other active modes. This is why random lasers and degenerate lasers are good candidates for producing low coherence light sources, they have many modes with similar *Q*-factors, whose spatial profiles are uniformly distributed throughout the cavity, effectively minimizing gain competition [26, 27, 31–33]. For comparison, perfectly circular disk lasers are a poor choice for a low-coherence laser. While disk cavities do support many high-*Q* modes, these are all whispering gallery modes and are localized at the edge of the cavity, which leads to large mode competition, such that only a few of these modes reach threshold.

The chaotic ray trajectories of the D-shaped cavities result in passive cavity resonances whose spatial profiles are relatively uniformly distributed across the cavity, leading to a narrow distribution of *Q* values and no very high Q modes with special geometry. Nonetheless, the high index mismatch at the boundary is sufficient to bring the lasing threshold into a reasonable range. Thus, optimizing multi-mode behavior in such a cavity depends upon reducing the effects of mode competition, which can be calculated exactly using SALT, and estimated with resonance SPA-SALT. In Fig. (1) we calculate the modal intensities (a)–(c), and generalized modal competition parameters, *λ* (d)–(f), using the passive cavity mode profiles compare this to full SALT simulations of the same cavity. Semi-quantitative agreement is seen between these two different computational methods, and both calculations independently agree on the geometry of the D-shaped cavity, *r*_{0} = .5*R*, which minimizes the effects of mode competition, and thus produces the most lasing modes for similar values of the pump. However, full SALT simulations of the cavity in this multi-mode regime require hundreds of hours of computational time to both generate the necessary CF basis states and solve the coupled non-linear equations above threshold, while the resonance SPA-SALT calculations require mere minutes after calculating the passive cavity resonances.

#### 3.2. Enhancing multi-mode behavior with non-uniform pumping

Having now demonstrated that resonance SPA-SALT agrees semi-quantitatively with the exact theory, one can use SPA-SALT as part of an optimization scheme to guide laser design. In this section, we explore the effects of non-uniform pumping on chaotic cavities to further increase their multi-mode behavior, and demonstrate that resonance SPA-SALT is compatible with existing non-linear optimization methods.

To begin, we consider a D-shaped cavity with independently tunable electrical contacts providing the current to the gain medium {*p _{i}*}, which yields a spatially inhomogeneous gain profile in Eq. (7). (We assume there is no significant gain diffusion in the medium.) These electrical contacts are segmented both angularly and radially, but together cover the entire cavity. Most non-linear optimization techniques work to minimize a fitness function with respect to an array of inputs, and so to optimize a pump profile for

*N*lasing modes we choose the fitness function,

_{L}*F*, to be

*N*= 10 lasing modes can be reduced by over a factor of 2.

_{L}#### 3.3. Reducing multi-mode behavior with non-uniform pumping

To demonstrate the flexibility of the pump optimization method for a given system, we now change our desired target for optimization, and try to inhibit multimode lasing through nonuniform pumping of a similar D-shaped cavity. This type of pump control has been demonstrated in previous work [3–6], although not with this method and not in such a highly multi-mode cavity as this. In Fig. 3, we show the modal intensities as a function of pump strength calculated using SALT (solid lines), and resonance SPA-SALT (dashed lines), where the passive cavity resonances have again been calculated using COMSOL Multiphysics. Here, we have chosen to use *r*_{0} = 0.5*R* to show that we can control the number of modes even for cavities with highly multimode behavior, but the results presented here are similar for other values of *r*_{0}. In the left panel of Fig. 3, we show the results for uniform pumping, wherein the first two lasing modes are seen to have similar thresholds, indicating that the effects of mode competition are weak.

However, as shown in the right panel of Fig. 3, by changing the pump profile of the cavity to have the same overall gain but an inhomogeneous distribution, the effects of mode competition can be increased, resulting in a substantially increased range of single mode operation. Here we have chosen to optimize the pump profile to promote single mode lasing while maintaining the same lasing threshold to facilitate switching between single-mode and multi-mode behavior. To do so, we are instead using a fitness function to both select for the same lasing threshold as the uniformly pumped cavity, while increasing the interacting threshold of the second mode relative to the first,

## 4. Summary

In conclusion, we have demonstrated that non-linear properties of above threshold lasers with *Q* > 100 can be calculated using knowledge of the passive cavity resonances and the resonance-based SPA-SALT equations. These results show semi-quantitative agreement with the full SALT simulations, for all of the semi-classical properties of lasers of interest, non-interacting and interacting modal thresholds, power slopes, and mode profiles. Using resonance SPA-SALT, we were then able to increase the multi-mode behavior of chaotic D-shaped cavities, demonstrating a potential role for selective pumping in the development of improved incoherent laser light sources. We note that, due to fabrication imperfections, often the goal of device optimization methods is to inform the experimental design process, not necessarily to achieve a highly accurate quantitative prediction for results. For the purpose of this type of exploratory device design, resonance SPA-SALT is able to provide the same insights as full SALT simulations, but using widely available software for resonance calculations in conjunction with an open source implementation of the method derived here.

## Funding

National Science Foundation (NSF) (DMR-1307632, ECCS1509361); Office of Naval Research (ONR) (MURI N00014-13-1-0649).

## References and links

**1. **N. Bachelard, J. Andreasen, S. Gigan, and P. Sebbah, “Taming random lasers through active spatial control of the pump,” Phys. Rev. Lett. **109**, 033,903 (2012). [CrossRef]

**2. **T. Hisch, M. Liertzer, D. Pogany, F. Mintert, and S. Rotter, “Pump-controlled directional light emission from random lasers,” Phys. Rev. Lett. **111**, 023902 (2013). [CrossRef] [PubMed]

**3. **L. Ge, O. Malik, and H. E. Türeci, “Enhancement of laser power-efficiency by control of spatial hole burning interactions,” Nat. Photonics **8**, 871–875 (2014). [CrossRef]

**4. **S. F. Liew, B. Redding, L. Ge, G. S. Solomon, and H. Cao, “Active control of emission directionality of semiconductor microdisk lasers,” Appl. Phys. Lett. **104**, 231,108 (2014). [CrossRef]

**5. **S. F. Liew, L. Ge, B. Redding, G. S. Solomon, and H. Cao, “Pump-controlled modal interactions in microdisk lasers,” Phys. Rev. A **91**, 043,828 (2015). [CrossRef]

**6. **L. Ge, “Selective excitation of lasing modes by controlling modal interactions,” Opt. Express **23**, 30,049 (2015). [CrossRef]

**7. **L. Ge, H. Cao, and A. D. Stone, “Condensation of thresholds in multimode microlasers,” arXiv:1607.08204, in submission.

**8. **B. Bidégaray, “Time discretizations for maxwell-bloch equations,” Numer. Meth. Partial Differential Equations **19**, 284–300 (2003). [CrossRef]

**9. **Y. Huang and S. Ho, “Computational model of solid-state, molecular, or atomic media for fdtd simulation based on a multi-level multi-electron system governed by pauli exclusion and fermi-dirac thermalization with application to semiconductor photonics,” Opt. Express **14**, 3569–3587 (2006). [CrossRef] [PubMed]

**10. **K. Böhringer and O. Hess, “A full-time-domain approach to spatio-temporal dynamics of semiconductor lasers. i. theoretical formulation,” Prog. Quantum Electron. **32**, 159–246 (2008). [CrossRef]

**11. **Y. Huang and S.-T. Ho, “Dynamical semiconductor medium FDTD simulation of current-injection nanophotonic devices,” Opt. Quantum Electron. **40**, 337–341 (2008). [CrossRef]

**12. **A. Cerjan, A. Pick, Y. D. Chong, S. G. Johnson, and A. D. Stone, “Quantitative test of general theories of the intrinsic laser linewidth,” Opt. Express **23**, 28,316–28,340 (2015). [CrossRef]

**13. **H. E. Türeci, A. D. Stone, and B. Collier, “Self-consistent multimode lasing theory for complex or random lasing media,” Phys. Rev. A **74**, 043,822 (2006). [CrossRef]

**14. **L. Ge, Y. D. Chong, and A. D. Stone, “Steady-state ab initio laser theory: generalizations and analytic results,” Phys. Rev. A **82**, 063,824 (2010). [CrossRef]

**15. **A. Cerjan, Y. D. Chong, and A. D. Stone, “Steady-state ab initio laser theory for complex gain media,” Opt. Express **23**, 6455–6477 (2015). [CrossRef] [PubMed]

**16. **S. Sunada, T. Fukushima, S. Shinohara, T. Harayama, and M. Adachi, “Stable single-wavelength emission from fully chaotic microcavity lasers,” Phys. Rev. A **88**, 013802 (2013). [CrossRef]

**17. **A. Cerjan, “Resonance SPA-SALT,” github (2016) [retrieved 26 August 2016], https://github.com/acerjan/comsol_spasalt.

**18. **J. U. Nöckel and A. D. Stone, “Ray and wave chaos in asymmetric resonant optical cavities,” Nature **385**, 45–47 (1997). [CrossRef]

**19. **C. Gmachl, F. Capasso, E. E. Narimanov, J. U. Nöckel, A. D. Stone, J. Faist, D. L. Sivco, and A. Y. Cho, “High-power directional emission from microlasers with chaotic resonators,” Science **280**, 1556–1564 (1998). [CrossRef] [PubMed]

**20. **H. Cao, Y. G. Zhao, S. T. Ho, E. W. Seelig, Q. H. Wang, and R. P. H. Chang, “Random laser action in semiconductor powder,” Phys. Rev. Lett. **82**, 2278–2281 (1999). [CrossRef]

**21. **H. Cao, “Review on the latest developments in random lasers with coherent feedback,” J. Phys. A **38**, 10497–10535 (2005). [CrossRef]

**22. **A. Sommerfeld, *Partial Differential Equations in Physics* (Academic Press, 1949).

**23. **S. Esterhazy, D. Liu, M. Liertzer, A. Cerjan, L. Ge, K. G. Makris, A. D. Stone, J. M. Melenk, S. G. Johnson, and S. Rotter, “Scalable numerical approach for the steady-state ab initio laser theory,” Phys. Rev. A **90**, 023816 (2014). [CrossRef]

**24. **A. Taflove and S. C. Hagness, *Computational Electrodynamics: The Finite-Difference Time-Domain Method* (Artech House, Incorporated, 2005).

**25. **A. Goetschy, A. Cerjan, and A. D. Stone, “Analytic statistical theory of random lasers in the non-linear regime,” in preparation.

**26. **B. Redding, M. A. Choma, and H. Cao, “Spatial coherence of random laser emission,” Opt. Lett. **36**, 3404–3406 (2011). [CrossRef] [PubMed]

**27. **B. Redding, M. A. Choma, and H. Cao, “Speckle-free laser imaging using random laser illumination,” Nat. Photonics **6**, 355–359 (2012). [CrossRef] [PubMed]

**28. **B. Redding, A. Cerjan, X. Huang, M. L. Lee, A. D. Stone, M. A. Choma, and H. Cao, “Low spatial coherence electrically pumped semiconductor laser for speckle-free full-field imaging,” Proc. Natl. Acad. Sci. U. S. A. **112**, 1304–1309 (2015). [CrossRef] [PubMed]

**29. **L. Bunimovich, “Ergodic properties of nowhere dispersing billiards,” Commun. Math. Phys. **65**, 295–312 (1979). [CrossRef]

**30. **S. Ree and L. Reichl, “Classical and quantum chaos in a circular billiard with a straight cut,” Phys. Rev. E **60**, 1607–1615 (1999). [CrossRef]

**31. **M. Nixon, B. Redding, A. A. Friesem, H. Cao, and N. Davidson, “Efficient method for controlling the spatial coherence of a laser,” Opt. Lett. **38**, 3858–3861 (2013). [CrossRef] [PubMed]

**32. **B. H. Hokr, J. N. Bixler, G. D. Noojin, R. J. Thomas, B. A. Rockwell, V. V. Yakovlev, and M. O. Scully, “Single-shot stand-off chemical identification of powders using random raman lasing,” Proc. Natl. Acad. Sci. U. S. A. **111**, 12320–12324 (2014). [CrossRef] [PubMed]

**33. **B. H. Hokr, M. S. Schmidt, J. N. Bixler, P. N. Dyer, G. D. Noojin, B. Redding, R. J. Thomas, B. A. Rockwell, H. Cao, V. V. Yakovlev, and M. O. Scully, “A narrow-band speckle-free light source via random Raman lasing,” arXiv: 1505.07156 (2015).