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A beam's transverse intensity changes its own refractive index. For positive nonlinear index and a bright centre, the accumulated phase has the curvature of a converging lens. For $I(r)=I_0{e}^{-2r^2/w^2}$ over a short length $L$, the in-medium thin-lens approximation gives $1/f=4n_2{I}_{0}L/(n_0{w}^2)$. Negative $n_2$ instead produces self-defocusing.

An intensity-dependent refractive index produced by the optical field itself. In a simple instantaneous isotropic model, $n=n_0+n_{2}I$. A transversely nonuniform intensity produces self-focusing for positive $n_2$ and self-defocusing for negative $n_2$. Temporal intensity variation produces self-phase modulation. These are consequences of a third-order nonlinear optical susceptibility, distinct from a static applied-field electro-optic Kerr effect.

A finite beam has an intensity gradient across its wavefront. In an instantaneous optical Kerr model, $n(r)=n_0+n_{2}I(r)$. A bright centre therefore sees a larger index for $n_2>0$, accumulating more phase than the wings and producing self-focusing. Negative $n_2$ gives self-defocusing. For a short medium and Gaussian $I(r)=I_0{e}^{-2r^2/w^2}$, expand the nonlinear phase near the axis:Compare with the in-medium thin-lens phase $-k{r}^2/(2f)$, where $k=n_0{k}_0$. The Kerr lens has $1/f=4n_2{I}_{0}L/(n_0{w}^2)$. This local quadratic fit describes the central lens, not the whole Gaussian phase or a guaranteed aberration-free focus.

Propagation combines diffraction with the nonlinear phase. Choose $|A{|}^2=I$ and a scalar paraxial envelope, givingThe diffraction length is of order $k{w}^2$, while the nonlinear length is $1/(|\gamma |I_0)$. Their competition depends on total beam power as well as spot size. In two transverse dimensions, balancing them gives a critical power scale $P_{\mathrm{cr}}\sim {\lambda }_0^2/(n_0{n}_2)$ for positive $n_2$; the numerical constant requires a specified transverse profile and critical solution. In the ideal unsaturated cubic model, sufficiently strong focusing can collapse rather than form a stable beam. Real saturation, absorption, ionization or nonparaxial propagation can stop that ideal singularity; the appropriate mechanism depends on the material and pulse regime.

A broad focusing beam can also break into filaments. Perturb the uniform solution $A_0{e}^{i\gamma I_{0}z}$ by real amplitude and phase components with transverse wave number $q$. Linearization gives the transverse modulational instability rateFor positive $\gamma$, modes with $0<q^2<4k\gamma I_0$ grow. diffraction suppresses very fine perturbations. A finite beam's boundaries and available propagation length limit which filaments develop. The defocusing sign has no growing band in this simple instantaneous local model.

A spatial optical soliton instead has a profile whose nonlinear focusing balances diffraction. A one-transverse-dimensional cubic focusing model supports a stationary bright solution; the existence of that solution does not establish robust two-dimensional cubic self-trapping. A beam can also act on another finite beam through cross-phase modulation, producing an induced lens or steering it towards a high-index region. Unequal polarization response can rotate or reshape the profile. Temporal self-phase modulation is a related consequence of a time-dependent intensity, but should be distinguished from these transverse effects.

For an experimental check, vary power at fixed input waist and compare near- and far-field profiles with a low-power diffraction reference. Repeat with a second beam blocked to separate cross-phase modulation from self-action. Vary pulse duration or repetition rate to test thermal lensing against a prompt electronic response, and monitor transmission to distinguish nonlinear refraction from preferential absorption. A smaller output spot alone does not establish a soliton or a pure Kerr response.