Generation of Bessel Surface Plasmon Polaritons in a Finite-Thickness Metal Film

Abstract

A theory of generation of low- and high-index Bessel surface plasmon polaritons and their superposition in a metal film of a finite thickness is developed. Correct analytical expressions are obtained for the field of two families of Bessel surface plasmon polariton modes formed inside and outside the metal layer. The intensity distribution near the boundary of the layer has been calculated and analyzed. A scheme for the experimental realization of a superposition of Bessel surface plasmon polaritons is suggested. Our study demonstrates that it is feasible to use the superposition of Bessel surface plasmon polaritons as a virtual tip for near-field optical microscopy with a nanoscale resolution.

1. Introduction

Surface plasmon polaritons (SPPs) are surface electromagnetic waves related to collective electron oscillations near the metal surface excited by light [1–3]. These fields arise under the resonance condition, and due to such nature of excitation, they are attractive in the context of enhancing the resolution of imaging systems substantially by increasing the amplitude of evanescent waves [4–6].

In 1987, Durnin et al. suggested a new type of waves, namely, Bessel light beams (BLBs), that kept the transverse spot size unchanged much longer than the Rayleigh range [7, 8]. Such a localized radiation mode was called the nondiffracting beam (or the diffraction-free beam). The transverse profile of the amplitude of this beam is described by a Bessel function of the first kind. In the domain of spatial frequencies, BLB is represented as a superposition of plane waves which are wrapped around a conical surface. Within the last decades, an intensive study of the scalar and vector BLBs has been made theoretically and experimentally (see, e.g., [9–18]). Bessel light beams are used in numerous applications, such as the optical manipulation of microsized particles [19], the fabrication of long polymer fiber induced by the photopolymerization [20] and microchanneling by structural modification in glass materials [21] the enhancement of energy gain in inverse-free electron lasers and inverse Cherenkov accelerators [22].

The authors of [23] pioneered in obtaining solutions of Maxwell’s equations which correspond to evanescent BLBs formed in the condition of the internal total reflection in an optically less dense dielectric medium. A more detailed theory of evanescent Bessel beams is presented in [24–29]. These beams exponentially decay while moving off the surface but retain their original transversal shape. In those investigations, of particular interest was the structure of the central lobe of evanescent BLBs. It is established that its diameter can be reduced to a nanosize value. This makes it possible to use evanescent Bessel beams in optical microscopy [30].

But the evanescent BLBs investigated before [24–29] possess an essential disadvantage, namely, they are weak, which causes the necessity of application of strong laser fields for their generation. One of the ways of taking Bessel light field advantages for microscopy is the formation of Bessel surface plasmon polaritons (BSPPs). Kano et al. [31] reported the first experimental result concerning an efficient excitation of surface plasmon polaritons by using the zeroth-order BLBs. More recently, radially polarized BLBs have been demonstrated to provide the TM polarization required for an effective coupling to the SPPs, which can be used as a virtual probe for the two-photon fluorescence microscopy [32]. In paper [33], the authors have demonstrated the existence of SPP in a multilayered metal-dielectric structure that evolves without distortion within an energy attenuation length and whose in-plane profile traces a Bessel function along the transverse direction relative to the beam axis.

However, despite of intensive theoretical and experimental investigations up to now there is no detailed analysis of the problem of generation of different types of Bessel surface plasmon polaritons in the structure including a metallic absorbing layer separating a substrate and targeted (dielectric) medium. Also of great interest is the study of the intensity distribution in the structure containing a thin metal film. An exact solution of these problems is presented in this paper.

The study of the superposition of two vortex Bessel surface plasmon polaritons with opposite topological charges (𝐽_𝑚 and 𝐽_−𝑚) is undoubtedly beneficial in practical terms. Such superposed beams are promising for creating near the interface an array of diffraction-free nanoscale light needles. At the same time, we attach importance to the development of a scheme for experimental realization of a superposition of Bessel surface plasmon polaritons. And the theory developed ought to be best suited to experiment. This practical motivation necessitates a more detailed description of the field which is a superposition of Bessel surface plasmon polaritons.

The paper is structured as follows. In Section 2, the description of features of generation of different types of Bessel surface plasmon polaritons in layered metal-dielectric structure is presented. The intensity distribution in the structure is analyzed in details analytically and numerically in Section 3. The possibility of the use of a superposition of Bessel surface plasmon polaritons is considered in Section 4. A conclusion is given in Section 5.

2. Description of Bessel Surface Plasmon Polaritons Generation in a Metal-Dielectric Layered Structure

2.1. Formation of Bessel Surface Plasmon Polaritons in a Finite-Thickness Metal Film

Let us consider a vector TM-polarized high-order (𝑚≠0) Bessel light beam 𝐽_𝑚 (BLB) incident onto the boundary of two semi-infinite media. We use the cylindrical coordinate system with the unit vectors 𝑒_𝜌,  𝑒_𝜑, and  𝑒_𝑧 (𝑒_𝑧 is collinear to the propagation direction). It is known (see, e.g., [10, 17, 18]) that the electric 𝐸(𝑅) and magnetic 𝐻(𝑅) vectors of BLB, propagating normally (in 𝑧-direction) in a medium with the refractive index 𝑛_𝑖, can be represented as 𝐸(𝑅)=𝐴𝐸^TM𝜌exp𝑖𝑘_𝑧𝑖,𝐻(𝑅)𝐻𝑧+𝑚𝜑=𝐴^TM𝜌exp𝑖𝑘_𝑧𝑖𝑧+𝑚𝜑, (1) where 𝑅=(𝜌,𝜑,𝑧) are the cylindrical coordinates, 𝑚 is an integer, 𝑘_𝑧𝑖 is the 𝑧-component of the wave vector, 𝐴 is a complex constant, the common phase multiplier exp[𝑖(𝑞𝑥−𝜔𝑡)] is omitted, and 𝑞=𝑘²₀𝑛_𝑖²−𝑘²_𝑧𝑖 is the transversal component of the wave vector.

Using the solution of Maxwell’s equations for the components of the vector amplitudes 𝐸^TM(𝜌),  𝐻^TM(𝜌), the problem of transmission and reflection of vector Bessel beams at the boundary of two dielectrics has been solved (see [17, 18]). Following [17, 18], in the case of TM-polarized BLB with an amplitude 𝐴_inc incident on the interface between two media characterized by refractive indices 𝑛_𝑖 and 𝑛_𝑗, the electric 𝐸_𝑡(𝑅) and magnetic 𝐻_𝑡(𝑅) vectors of the refracted Bessel beam (symbol “𝑡” denotes refracted BLB) can be represented in the form 𝐸_𝑡(𝑅)=𝐸_𝑡^tr(𝑅)+𝐸^𝑙_𝑡(𝑅),𝐸^𝑙_𝑡(𝑅)=𝐴_inc𝑡^TM_𝑖𝑗exp𝑖𝑚𝜑+𝑘_𝑧𝑗𝑧sin𝛾_𝑗𝐽_𝑚𝑞𝜌𝑒_𝑧,𝐸_𝑡^tr(𝑅)=𝑖𝐴_inc√2exp𝑖(𝑚−1)𝜑+𝑘_𝑧𝑗𝑧𝑡^TM_𝑖𝑗×cos𝛾_𝑗𝐽_𝑚−1𝑞𝜌𝑒₊−𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋,𝐻_𝑡(𝑅)=𝑛_𝑗𝐴_inc√2exp𝑖(𝑚−1)𝜑+𝑘_𝑧𝑗𝑧𝑡^TM_𝑖𝑗×𝐽_𝑚−1𝑞𝜌𝑒₊+𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋. (2)(3) Here cos𝛾_𝑗=𝑘_𝑧𝑗/𝑘₀𝑛_𝑗,𝑘₀=𝜔/𝑐, 𝜔 is the frequency of the Bessel beam, 𝑐 is the light velocity in vacuum, 𝐽_𝑚(𝑞𝜌) is the 𝑚-order Bessel function; symbols “tr,” “𝑙” denote the transversal and longitudinal component of the electric (magnetic) vector, respectively; 𝑡^TM_𝑖𝑗=𝐴^TM_𝑡/𝐴_inc is the amplitude transmission coefficient; 𝐴^TM_𝑡 is the amplitude factor for TM BLB; 𝑒_±=(𝑒₁±𝑖𝑒₂)/√2 are the unit circular vectors which are orthogonal to the 𝑒_𝑧 vector.

In a similar manner, for the reflected field (it is marked with the symbol “𝑟”), we obtain 𝐸_𝑟(𝑅)=𝐸_𝑟^tr(𝑅)+𝐸^𝑙_𝑟(𝑅),𝐸^𝑙_𝑟(𝑅)=𝐴_inc𝑟^TM_𝑖𝑗exp𝑖𝑚𝜑−𝑘_𝑧𝑖𝑧sin𝛾_𝑖𝐽_𝑚𝑞𝜌𝑒_𝑧,𝐸_𝑟^tr(𝑅)=−𝑖𝐴_inc√2exp𝑖(𝑚−1)𝜑−𝑘_𝑧𝑖𝑧𝑟^TM_𝑖𝑗×cos𝛾_𝑖𝐽_𝑚−1𝑞𝜌𝑒₊−𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋,𝐻_𝑟(𝑅)=𝑛_𝑖𝐴_inc√2exp𝑖(𝑚−1)𝜑−𝑘_𝑧𝑖𝑧𝑟^TM_𝑖𝑗×𝐽_𝑚−1𝑞𝜌𝑒₊+𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋. (4)(5) Here 𝑟^TM_𝑖𝑗=𝐴^TM_𝑟/𝐴_inc is the amplitude reflection coefficient; 𝐴^TM_𝑟 is the amplitude factor for TM BLB. The amplitude refraction and reflection coefficients are 𝑡^TM_𝑖𝑗=2𝑛_𝑖cos𝛾_𝑖𝑛_𝑖cos𝛾_𝑗+𝑛_𝑗cos𝛾_𝑖,𝑟^TM_𝑖𝑗=𝑛_𝑗cos𝛾_𝑖−𝑛_𝑖cos𝛾_𝑗𝑛_𝑗cos𝛾_𝑖+𝑛_𝑖cos𝛾_𝑗. (6) Equations (6) can be used for the description of the transformation of BLB at the boundary between dielectric with the real refractive index 𝑛_𝑖 and metal having the complex refractive index 𝑛_𝑗=𝑛^′_𝑗+𝑖𝑛_𝑗^′′, where 𝑛^′_𝑗=Re(𝑛_𝑗),𝑛_𝑗^′′=Im(𝑛_𝑗).

Using (2), (3), and (6), let us consider now the formation of Bessel surface plasmon polaritons in a layered structure containing a metal film with the dielectric constant 𝜀₁=𝑛²₁ and thickness ℎ between two semi-infinite dielectric media with dielectric constants 𝜀₀=𝑛²₀,𝜀₂=𝑛²₂ (Figure 1). The origin of the coordinated system 𝑧=0 is assumed to be chosen at the interface between the dielectric substrate and the layer 𝜀₁ (Figure 1).

Figure 1 

Schematic representation of the structure including a metallic layer (𝜀1), a substrate (𝜀0), and a targeted (𝜀2) medium.

In view of (2), (4), the electric vector of the field inside the metal layer and outside it is expressed as𝐸₀(𝑅)=𝐸₀^tr(𝑅)+𝐸^𝑙₀(𝑅),𝐸^𝑙₀(𝑅)=𝐴_inc𝑞𝑘₀𝑛₀exp𝑖𝑚𝜑−𝑘_𝑧0𝑧𝐽_𝑚𝑞𝜌𝑒_𝑧,𝐸₀^tr(𝑅)=−𝑖𝐴_inc√2exp𝑖(𝑚−1)𝜑−𝑘_𝑧0𝑧×𝑞1−𝑘₀𝑛₀²𝐽_𝑚−1𝑞𝜌𝑒₊−𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋,𝐸₂(𝑅)=𝐸₂^tr(𝑅)+𝐸^𝑙₂(𝑅),𝐸^𝑙₂(𝑅)=𝐴_inc𝑞𝑘₀𝑛₂𝑡exp𝑖𝑚𝜑+𝑘_𝑧2(𝑧−ℎ)𝐽_𝑚𝑞𝜌𝑒_𝑧,𝐸₂^tr(𝑅)=𝑖𝐴_inc√2exp𝑖(𝑚−1)𝜑+𝑘_𝑧2(𝑡×𝑧−ℎ)𝑞1−𝑘₀𝑛₂²𝐽_𝑚−1𝑞𝜌𝑒₊−𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋,𝐸₁(𝑅)=𝐸₁^tr(𝑅)+𝐸^𝑙₁(𝑅),𝐸^𝑙₁(𝑅)=𝐸^𝑙₁^𝑓+𝐸^𝑙₁^𝑏,𝐸₁^tr(𝑅)=𝐸₁^tr𝑓+𝐸₁^tr𝑏,𝐸^𝑙₁^𝑓,𝑏=𝐴_inc𝑞𝑘₀𝑛₁𝑠^𝑓,𝑏exp𝑖𝑚𝜑±𝑘_𝑧1𝑧𝐽_𝑚𝑞𝜌𝑒_𝑧,𝐸₁^tr(𝑅)^𝑓,𝑏=±𝑖𝐴_inc√2𝑠^𝑓,𝑏exp𝑖(𝑚−1)𝜑±𝑘_𝑧1𝑧×𝑞1−𝑘₀𝑛₁²𝐽_𝑚−1𝑞𝜌𝑒₊−𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋. (7a)(7b)

Here, symbols “0”, “1”, and “2” denote the substrate, metal layer, and targeted medium, respectively. Similarly, for the magnetic vector we have𝐻₀(𝑅)=𝑛₀𝐴_inc√2exp𝑖(𝑚−1)𝜑−𝑘_𝑧0𝑧×𝐽_𝑚−1𝑞𝜌𝑒₊+𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋,𝐻₂(𝑅)=𝑛₂𝐴_inc√2exp𝑖(𝑚−1)𝜑+𝑘_𝑧2(𝐽𝑧−ℎ)×𝑡_𝑚−1𝑞𝜌𝑒₊+𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋,𝐻₁(𝑅)=𝐻₁(𝑅)^𝑓+𝐻₁(𝑅)^𝑏,𝐻₁(𝑅)^𝑓,𝑏=𝑛₁𝐴_inc√2𝑠^𝑓,𝑏exp𝑖(𝑚−1)𝜑±𝑘_𝑧1𝑧×𝐽_𝑚−1𝑞𝜌𝑒₊+𝐽_𝑚+1𝑞𝜌exp2𝑖𝜑𝑒₋. (8a)(8b)Here, 𝑡=𝐴₂/𝐴_inc, 𝑠^𝑓=𝐴_𝑓/𝐴_inc, 𝑠^𝑏=𝐴_𝑏/𝐴_inc are the amplitude coefficients for the forward and backward Bessel fields inside the metal film, respectively; 𝐴_𝑓,𝑏 are the amplitude factors inside the metal layer.

Using the boundary conditions of continuity of the tangential components of the electric and magnetic fields, which have to be satisfied at the planes 𝑧=0 and 𝑧=ℎ, as well as (7a), (7b), (8a), (8b), and (6), we obtain the system of equations for the coefficients 𝑡,𝑠^𝑓,𝑏. As a result of its solution, one can find the dispersion equation determining the existence of Bessel surface plasmon polaritons in the structure shown in Figure 1: 1+𝑟^TM₀₁𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ=0. (9)

As known (see [34]), the amplitude reflection coefficient of the layer is 𝑟𝑟=^TM01+𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ1+𝑟^TM₀₁𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ. (10) Then, (9) determines the poles of the reflection coefficient 𝑟 of the metal layer. Taking into account (6), this expression can be transformed to the form 𝐹=−𝑖𝑡𝑔𝑘_𝑧1ℎ𝑘1+^2𝑧1𝜀₀𝜀₂𝑘_𝑧0𝑘_𝑧2𝜀²₁+𝑘_𝑧1𝜀₀𝑘_𝑧0𝜀₁+𝑘_𝑧1𝜀₂𝑘_𝑧2𝜀₁=0. (11)

Here, 𝑘_𝑧𝑖 is the 𝑧-component of the wave vector, and the index 𝑖 refers to the medium number. As seen from (11), unlike plane waves, the dispersion equation relates the frequency with the transversal component 𝑞=𝑘²₀𝑛_𝑗²−𝑘²_𝑧𝑗 of a Bessel surface plasmon polariton. Due to complexity of the metal refractive index, 𝑞 is a complex quantity. Here, Re𝑞 determines the radius of rings of the excited Bessel surface plasmon polariton.

The boundary conditions allow one to determine the quantities 𝑡,𝑠^𝑓, and  𝑠^𝑏 entering into (7a), (7b), (8a), and (8b): 𝑡𝑡=^TM01𝑡^TM₁₂exp𝑖𝑘_𝑧1ℎ1+𝑟^TM₀₁𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ,𝑠^𝑓=𝑡^TM₀₁1+𝑟^TM₀₁𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ,𝑠^𝑏=𝑡^TM₀₁𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ1+𝑟^TM₀₁𝑟^TM₁₂exp2𝑖𝑘_𝑧1ℎ. (12) Here, the coefficients 𝑡^TM_𝑖𝑗,𝑟^TM_𝑖𝑗 are determined by (6).

Then, (7a), (7b), (8a), (8b), and (12) at 𝑞, which meets condition (11), describe Bessel surface plasmon polaritons formed in the structure “dielectric substrate metal layer dielectric.” The field of a superposition of Bessel surface plasmon polaritons can be defined as a sum of the beams with the electric (magnetic) vector in the form (7a), (7b) ((8a), and (8b)).

It would be interesting to give a physical interpretation of the Bessel SPPs being localized and to compare them with traditional surface plasmon polaritons. It is well-known that the traditional SPPs are associated with the propagating wave process on metal/dielectric surface. In contrast to this, according to (7a), (7b), (8a), and (8b), the Bessel SPP is excited by an incident BLB, which can be considered as a superposition of 𝑝-polarized plane monochromatic waves having frequency 𝜔 and wave vectors lying on the surface of a cone.

The SPP propagating in the metal film is excited by every 𝑝-polarized plane-wave component of the incident BLB in conditions of the plasmon resonance. Here, the phase of every SPP is determined by the phase of the plane-wave component of the incident BLB. Thus, in the metal film, an array of propagating SPPs arises, wave vectors of which are being oriented in the direction of the center determining the intersection of the incident BLB axis with the surface of the metal film. As a result, there occurs the generation of pairs of two counter-propagating SPP waves with the wave vectors ±𝑞. The generated SPPs will propagate in all the possible radial directions to form a localized SPP field. This results in a complex high-symmetric interference light structure emerging in sections parallel to the metal-dielectric surface.

For the case where the longitudinal components of the electric field 𝐸^𝑙₁ for every radially propagating SPP has the same phase, in the center of such a standing light structure a maximum appears, that is, the shape of the 𝐸^𝑙₁ component of localized Bessel SPP is described by zero-order Bessel function 𝐽₀(𝑞𝜌). In a special case, each pair of counter propagating SPPs is in counter-phase and the local plasmonic field appears with a minimum in the center, that is, the so-called vortex localized Bessel SPP is formed. In this case, the electric field 𝐸^𝑙₁ of vortex Bessel SPP is described by 𝐽_𝑚(𝑞𝜌) Bessel function (see (7b)).

The problem should be studied now of attenuation of the Bessel SPP inside the metal layer. With this aim, the limited narrow Bessel light beam of radius 𝑟₀ in the transversal section should be considered. Such an apertured beam excites Bessel SSP in a cylindrical region limited by 𝑟₀. As follows from (7a), (7b), the transversal distribution of the longitudinal component of the electric field of Bessel SPP is determined by 𝐽_𝑚(𝑞𝜌) Bessel function which can be represented as a sum of the cylindrical Hankel functions of the first 𝐻_𝑚⁽¹⁾(𝑞𝜌) (outgoing) and second 𝐻_𝑚⁽²⁾(𝑞𝜌) (incoming) kinds [35]: 𝐽_𝑚=𝐻𝑞𝜌^𝑚(1)𝑞𝜌+𝐻_𝑚⁽²⁾𝑞𝜌2. (13)

According to (13), in the region 𝜌<𝑟₀, the Bessel SPPs are formed by converging and diverging conical beams described by appropriate Hankel functions. Outside the area 𝜌>𝑟₀ there exists only a diverging conical beam, and that is why in the decomposition (13) it is supposed that 𝐻_𝑚⁽²⁾=0. Using the asymptotic approximation of Hankel function [36], we obtain that the intensity of the longitudinal component of Bessel SPP electric vector |𝐸^𝑙|²∼|𝐽²_𝑚(𝑞𝜌)|² is determined by the expression 𝐸^𝑙2∼1𝑞²𝜌²exp−2Im𝑞𝜌. (14)

Thus, from (14), it follows that beyond the boundary of the exciting source the Bessel SPP decays exponentially in the radial direction. The 1/𝑒 energy-attenuation radius 𝑅_BSSP is determined by the imaginary part of the SPP wave number and given by the expression 𝑅_BSSP=1.2Im𝑞 (15) Thus, the energy-attenuation radius of Bessel SPP, generated by limited narrow Bessel beam, coincides with the decay length 𝐿_SP of propagating surface plasmon. From the physical point of view, it is explained by the fact that the Bessel SPP (outside the area of excitation) can be represented by the superposition of radially propagating plane wave SPPs.

2.2. Formation of Bessel Surface Plasmon Polaritons in a Symmetric Metal-Dielectric Layered Structure

Finding the roots of the complex equation (11) is numerically challenging. The reflection pole method (RPM) provides the phase of 𝐹 as a function of the real part of the Bessel surface plasmon polariton mode effective index 𝑛^∗=𝑞/𝑘₀. The Bessel surface plasmon polaritons correspond to the rapid changes of the phase of 𝐹 function. According to the Bode plot theory [37], a peak of the derivative of the phase of 𝐹 function corresponds to the real part of the Bessel surface plasmon polariton mode effective index, and the full width at the half maximum of the phase derivative curve is the imaginary part of the Bessel surface plasmon polariton mode effective index.

Using the reflection pole method, we searched the Bessel surface plasmon polaritons for a gold (Au) metal film (𝜀₁=−11.679+1.181𝑖 at the 0.633 micron wavelength [38]) of 50 nm thickness embedded in SF10 glass (𝜀₀=𝜀₂=(1.723)²). Figures 2(a) and 2(b) are the plots of the phase of 𝐹 function and its derivative versus the real part of the Bessel surface plasmon polariton mode effective index. From Figures 2(a) and 2(b), we see two rapid changes of the phase of 𝐹 which correspond to two Bessel surface plasmon polariton modes. The complex Bessel surface plasmon polariton mode effective indices we found are 𝑛^∗₁=1.874+0.012𝑖 and 𝑛^∗₂=2.179+0.073𝑖.

(a)

(b)

Figure 2 

The phase of 𝐹 function (a) and the derivative of the phase of 𝐹 function (b) versus the real part of the Bessel surface plasmon polariton mode effective index.

The first (so-called low-index Bessel surface plasmon polariton (LIBSPP)) and the second (high-index Bessel surface plasmon polariton (HIBSPP)) BSPPs are characterized by the first ring radius 𝑅₁≈2.4/(𝑘₀Re𝑛^∗)equal to 129 nm and 110 nm, respectively.

It is interesting to consider the symmetry of the longitudinal (𝐸^𝑙₁=𝐸^𝑙₁𝑒_𝑧) and transversal, for example, radial (𝐸^𝜌₁) components of the BSPP electric vector inside the metal layer. Note that the equation for 𝐸^𝜌₁ can be obtained from (7b). As calculation shows, the symmetry of real and imaginary parts of longitudinal (as well as transversal) components of electric vector of Bessel SPP inside the metal layer is the same. Figure 3 illustrates the dependence of the function Re𝐸^𝑙₁ normalized to the amplitude factor 𝐴_inc (at the center 𝜌=0 of Bessel surface plasmon polariton) on the distance 𝑧 in a 50 nm thickness gold film surrounded by dielectric media for low- and high-index zero-order BSPPs. It is seen that for the low-index Bessel SPP with the topological charge 𝑚=0, the distribution of 𝐸^𝑙₁(𝐸^𝜌₁) turns out to be symmetrical (antisymmetrical) (Figure 3) with respect to the middle plane of the metal film. For the high-index Bessel SPP, it is antisymmetrical (symmetrical).

(a)

(b)

Figure 3 

The normalized real part of the longitudinal 𝐸𝑙1 (a) and radial 𝐸𝜌1 (b) components of the electric vector for low-index (1) and high-index (2) TM-polarized zero-order Bessel surface plasmon polaritons versus the distance inside the gold film of 50 nm thickness embedded in SF10 glass. The distance from the Bessel surface plasmon polariton axis is 𝜌=0.05𝜇m, and the wavelength is 𝜆=0.633𝜇m.

Figure 4 demonstrates a 2D-pattern of the normalized intensity distribution |𝐸^𝑙₂|²/|𝐸^𝑙₂|²_max for low- and high-index Bessel surface plasmon polaritons formed outside the gold layer of 50 nm thickness embedded in SF10 glass. This is the most interesting case where BSPPs are generated by a purely radially polarized Bessel beam. The results of calculations presented in Figure 4 prove that the widths of the central maximum in the transverse distribution, which can be estimated approximately by the ratio 𝐷₁=2𝑅₁=4.8/(𝑘₀Re(𝑛^∗)), for LIBSPP as well as for HIBSPP, turn out to be less than the wavelength. It should be noted that as follows from (7a) while increasing the distance from the surface of the metal layer, the central peak of BSPP, generated in the structure, decays as exp(−Im𝑘_𝑧𝑖𝑧)(𝑖=1,2), but its transversal size 𝐷₁ does not change practically.

(a)

(b)

Figure 4 

2D pattern of normalized intensity distribution |𝐸𝑙2|2/|𝐸𝑙2|2max for low- (a) and high-index (b) zero-order Bessel surface plasmon polaritons outside the gold layer of 50 nm thickness embedded in SF10 glass. BSPPs are generated by a purely radially polarized Bessel beam having a wavelength of 633 nm. The distance from the entrance surface of the metal layer is 𝑧=𝜆/3.

Let us investigate now how the conditions of excitation of Bessel surface plasmon polaritons depend on the thickness of the metal layer. Figure 5 shows the dependence of the derivative of the phase of 𝐹 function versus the real part of the Bessel surface plasmon polariton mode effective index at various thicknesses of the gold film. It is seen that at an increase in the metal layer thickness two maxima of the curve merge into one, which testifies the degeneration of Bessel surface plasmon polariton modes. Here, the Bessel surface plasmon polariton mode effective index approaches the 𝑛^∗_free for the case of BSPP excitation at the boundary of two semi-infinite media—dielectric and metal [38]: 𝑛^∗_free=𝜀₂𝜀^′₁𝜀^′₁+𝜀₂+𝜀₁^′′2+𝑖𝜀₁^′′𝜀^′₁+𝜀₂−𝜀^′₁𝜀₁^′′𝜀^′₁+𝜀₂²+𝜀₁^2′′, (16) where 𝜀^′₁=𝑛₁^′2−𝑛₁^′′2, 𝜀₁^′′=2𝑛^′₁𝑛₁^′′. Equation (16) can be obtained from dispersion equation (11) at ℎ=0.

Figure 5 

The derivative of the phase of 𝐹 function versus the real part of Bessel surface plasmon polariton mode effective index for gold film of 100 nm (—), 80 nm (- - -), 60 nm (⋯), and 50 nm (·-·-·-) embedded in SF10 glass.

At a decrease in thickness of the metal film, the difference between the Bessel surface plasmon polariton mode effective indices increases. So, for example, in the structure containing gold (Au) metal film of 20 nm thickness embedded in SF10 glass, the effective indices take on the values 𝑛^∗₁=1.759+0.0018𝑖 and 𝑛^∗₂=3.212+0.234𝑖. At a metal film thickness of 15 nm, we have 𝑛^∗₁=1.744+0.0009𝑖 and 𝑛^∗₂=3.940+0.331𝑖. As is seen, in the first case the generated high-index Bessel surface plasmon polariton has the first ring radius 𝑅₁ equal to 75 nm. In the second case, while decreasing the thickness of metal film by 15 nm, it is possible to obtain HIBSPP with 𝑅₁≈61 nm.

Taking into account that 𝜀₁^′′ is significantly less than |𝜀^′₁|, (16) enables one to get the expressions for the real (𝑛^∗′_free) and imaginary (𝑛^∗′_free) parts of the effective index 𝑛^∗_free for Bessel surface plasmon polariton mode exited at the boundary of two semi-infinite media-dielectric and metal: 𝑛^∗′_free=𝜀^′₁𝜀₂𝜀^′₁+𝜀₂,𝑛^∗′′_free=𝜀^′₁𝜀₂𝜀^′₁+𝜀₂³𝜀₁^′′2𝜀^′₁². (17) The calculation, made according to (17), shows that for Bessel surface plasmon polariton, formed at the boundary of two semi-infinite media “gold-SF10 glass,” 𝑛^∗′′_free=0.034. As established above, for the structure containing the 50 nm thickness gold film embedded in SF10 glass, Im(𝑛^∗₁)=0.012. Thus, in a thin metal film immerged in a dielectric, there may be the generation of a low-index Bessel surface plasmon polariton, for which the imaging part of the Bessel surface plasmon polariton mode effective index appears to be lower than that for BSPP excited at the boundary of semi-infinite media “metal-dielectric.”

As it is mentioned above, in the 𝑧-direction, the electric field of the Bessel surface plasmon polariton decays as ∝exp(−Im𝑘_𝑧𝑖𝑧)(𝑖=0,1,2). The penetration depth of the field in the medium is determined by the expression 𝑑=1/Im𝑘_𝑧𝑖. As the calculation shows, for the LIBSPP penetration depth 𝑑_LIBSPP into the targeted medium turns out to be larger than 𝑑_free for the case of the plasmon formation at the “metal-dielectric” boundary. So, in the case under study 𝑑_LIBSPP=137nm, 𝑑_free=75nm.

Now using the reflection pole method, we consider the Bessel surface plasmon polaritons generation for a gold film of 50 nm thickness embedded in material for which the difference |𝜀₁|−𝜀₀ is lower than that in the case studied earlier. Such parameters belong, for example, to ZrO₂ (𝜀₀=𝜀₂=4). Figure 6 is the derivative of the phase of 𝐹 function versus the real part of the Bessel surface plasmon polariton mode effective index for this case. We see that there are two fast changes of the phase of 𝐹 corresponding to two Bessel surface plasmon polariton modes with the effective indices dependent on the thickness ℎ of the metal layer. As it follows from Figure 7, for ℎ=50 nm, we have 𝑛^∗₁=2.270+0.027𝑖 and 𝑛^∗₂=2.732+0.120𝑖; for ℎ=30 nm, we obtain 𝑛^∗₁=2.1320+0.0097𝑖 and 𝑛^∗₂=3.312+0.217𝑖; for ℎ=20 nm, we find 𝑛^∗₁=2.065+0.004𝑖 and 𝑛^∗₂=4.235+0.351𝑖. It is seen that if the difference between the dielectric constants of a targeted medium (substrate) and metal decreases, the Bessel surface plasmon polariton mode effective indices increase. Moreover, if ℎ decreases, the difference Δ𝑛^∗=𝑛^∗₂−𝑛^∗₁ increases. Thus, in a thin metal layer with a symmetric dielectric surrounding, the generation of a Bessel surface plasmon polariton with the first ring radius of several tens of nanometers is possible (see Figure 7).

Figure 6 

The derivative of the phase of 𝐹 function versus the real part of Bessel surface plasmon polariton mode effective index for the gold film of 50 nm (—), 30 nm (- - -), and 20 nm (⋯) embedded in ZrO2.

Figure 7 

Dependence of the first ring radius of Bessel surface plasmon polariton on the thickness of Au layer embedded in ZrO2 for high-index BSPP.

2.3. Formation of Bessel Surface Plasmon Polaritons in Metal Film with Asymmetric Dielectric Surrounding

The asymmetric configuration leads to more interesting phenomena. Using the reflection pole method for solving dispersion equation (11), we searched the Bessel surface plasmon polaritons for a gold metal film of 50 nm thickness separating SF10 glass and air. The complex Bessel surface plasmon polariton mode effective indices are found to be 𝑛^∗₁=1.0480+0.0001𝑖 and 𝑛^∗₂=2.022+0.043𝑖. Here, the profile of 𝐸^𝑙₁(𝑧) changes essentially inside the metal film for both generated types of TM₀ Bessel surface plasmon polaritons (Figure 8), that is, it losses symmetry with respect to the middle plane of the metal layer. Moreover, Figure 8 shows that there is a certain value 𝑧_𝑒 on the BSPP axis (𝜌=0), for which the longitudinal component of electrical vector 𝐸^𝑙₁ of high-index BSPP is equal to zero, in this concrete case 𝑧_𝑒=45 nm.

(a)

(b)

Figure 8 

The normalized real part of the longitudinal component 𝐸𝑙1 of electric vector of low-index (1) and high-index (2) TM0 Bessel surface plasmon polariton versus the distance inside the 50 nm gold film separating the SF10 glass and air (a) or fluid with refractive index 1.33 (b). The distance from the Bessel surface plasmon polariton axis is 𝜌=0, and the wavelength is 𝜆=0.633𝜇m.

As a result of the calculation performed with the help of the reflection pole method for solving dispersion equation (11), it is revealed that at an increase in the refraction index of the targeted medium Bessel surface plasmon polariton mode effective indices increase too, but their difference is determined, mainly, by the thickness of the metal film. And the value 𝑧_𝑒 decreases.

3. Intensity Distribution of Superposition of Bessel Surface Plasmon Polaritons in Layered Metal-Dielectric Structure

Let us consider now the intensity distribution of the superposition of two TM_𝑚 Bessel surface plasmon polaritons with different topological charges (𝑚₁≠𝑚₂) and phase changes (Δ₁≠Δ₂) inside the targeted medium: 𝐼∼𝐸^𝑙(𝑅)²,𝐸^𝑙(𝑅)=𝐴_inc𝑘₀𝑛₂×𝑞₁𝑡₁×𝑚exp𝑖₁𝜑+𝑘⁽¹⁾_𝑧2𝑧−ℎ₁+Δ₁𝐽_𝑚1𝑞₁𝜌+𝑞₂𝑡₂exp𝑖𝑚₂𝜑+𝑘⁽²⁾_𝑧2𝑧−ℎ₁+Δ₂×𝐽_𝑚2𝑞₂𝜌𝑒_𝑧. (18) Here, parameters 𝑡₁,  𝑡₂ determine the amplitudes of interfering plasmons and can be calculated from (12), 𝑘^(1,2)_𝑧2=𝑘²₀𝑛²₂−𝑞²_1,2. We will consider in more detail the case of practical interest where Bessel surface plasmon polaritons are generated in a Au film separating SF10 glass and air. This case is described in Section 2.3. Two different variants are realizable: case 1 where BSPPs with different 𝑛^∗ (and hence, 𝑞) interfere; case 2 when BSPPs with equal 𝑛^∗ (and hence, 𝑞) but different topological charges and/or phase changes interfere. Now consider one more important case where interfering Bessel surface plasmon polaritons with the same mode effective indices have topological charges equal in value but different in sign. In this case, the superposition of two BSPPs 𝐽_𝑚 and 𝐽_−𝑚, leads to the excitation of Bessel surface multiplasmon polariton for which, as it follows from (18), the azimuthal modulation of intensity is brought about. Owing to this, the interference structure being a set of annular maxima is separated into substructures at a nanoscale transverse size. Figure 9 illustrates the 2D distribution of normalized intensity in the air at the distance 𝑧=𝜆/3 μm from the boundary with metal layer. Here, the plasmon polariton field is a superposition of 𝐽₃ and 𝐽₋₃ low-index (a) and high-index (b) BSPPs. Figures 9(c) and 9(d) show that the field formed by two interfering high-index Bessel surface plasmon polaritons is characterized by more narrow near-axial maxima and essential suppression of lateral maxima while moving off the field axis to its periphery. The above-mentioned interference patterns are rather stable when moving off the interface of metal film. In Figure 10, as an example, the 2D normalized intensity distribution of the field formed by 𝐽₃ and 𝐽₋₃ low-index BSPPs is given at various distances from the “metal-air” boundary.

(a)

(b)

(c)

(d)

Figure 9 

2D and 3D normalized intensity distribution |𝐸𝑙2|2/|𝐸𝑙2|2max of Bessel multiplasmon in the air at the distance 𝑧=𝜆/3 μm from the interface of 50 nm thickness gold film of “SF10 glass—Au layer—air” structure. Bessel surface multiplasmon polariton is a superposition of 𝐽3 and 𝐽−3 low-index (a, c) and high-index (b, d) BSPPs with wavelength 𝜆=0.633 μm.

(a)

(b)

(c)

Figure 10 

2D normalized intensity distribution |𝐸𝑙2|2/|𝐸𝑙2|2max of Bessel surface multiplasmon polariton in the air at the distance 𝑧=𝜆/3μm (a), 𝑧=𝜆/2 μm (b), and 𝑧=𝜆 μm (c) from the interface of 50 nm thickness gold film of “SF10 glass—Au layer—air” structure. Bessel surface multiplasmon polariton is a superposition of 𝐽3 and 𝐽−3 low-index BSPPs with wavelength 𝜆=0.633 μm.

Thus, the superposition of two oppositely charged Bessel surface plasmon polaritons allows one to form near the interface of metal an array of quasi-nondiffracting nanoscale spots.

4. Possible Applications of a Superposition of Bessel Surface Plasmon Polaritons

Thus, the established property of a superposition of Bessel surface plasmon polaritons is applicable to the creation of a virtual multitip for near-field optics. A conceptual sketch of formation of such a multitip, the so-called virtual Bessel surface multiplasmon polariton tip, is illustrated in Figures 11 and 12.

Figure 11 

Schematic set-up for excitation of Bessel surface multiplasmon polariton. 1 and 1′ are extreme rays of conical beams excited Bessel surface plasmon polaritons, and 2 is conical lens on the basic surface of which metal film 3 is plotted.

Figure 12 

Basic scheme of obtaining of conical beams. RCL is a reflective conical lens, CM is a conical mirror, 1 and 1′ are extreme rays of the formed conical beam.

As is seen from Figure 11, the lateral surface of conical lens 2 is illuminated by two conical beams (their extreme rays 1 and 1′ are presented in Figure 11) having the same half-cone angles. These beams are necessary for further exiting BSPPs. One of the pointed conical beams is obtained from the TM_𝑚 Bessel mode, and another conical beam is formed from the TM_−𝑚 BLB using a scheme represented in Figure 12 [39] and composed of a reflective conical lens (RCL) and conical mirror (CM). Both conical beams incident on the conical lens 2 perturb Bessel surface plasmon polaritons in metallic film 3. In the region of overlapping of conical beams (shaded area in Figure 11), a superposition of two Bessel surface plasmon polaritons is generated. In turn, in the air near the base surface of the conical lens covered by metal layer 3, a Bessel surface multiplasmon polariton is formed. If the tested surface is placed at the distance 𝑧≤𝜆 from the metal layer, the forming exponentially decaying field penetrates into the surface. Thus, the superposition of Bessel surface plasmon polaritons can be used for testing the surfaces of various specimens.

The first crucial advantage of the near-field technique based on a superposition of Bessel surface plasmon polaritons is related to the nondiffractional nature of these fields. Namely, the virtual Bessel surface multiplasmon polariton tip is characterized by the constant size of a probing beam while increasing the probe-to-sample distance which can vary from zero up to ∼𝜆. Thus, the use of the virtual Bessel surface multiplasmon polariton tip allows one to extend potentially the working distance between an object and apparatus.

The important feasible application of beams under consideration is also creating multiple optical traps when using two interfering high-order Bessel surface plasmon polaritons.

5. Conclusion

In this paper, a theory is developed of the generation of single Bessel SPPs and their superposition in the structure including a metal layer separating two semi-infinite dielectrics.

The comparison was made of Bessel surface plasmon polaritons investigated in this paper and traditional surface plasmon polaritons. The traditional SPP is a propagating wave process on the metal/dielectric surface. Unlike it, Bessel SPP is a superposition of counter propagating SPPs in all the possible radial directions. It is a complex high-symmetric interference light structure in sections parallel to the metal/dielectric interface. It should be noted as opposed to the propagating surface plasmon polariton, the Bessel one is a standing light structure.

The problem is studied of attenuation of the Bessel SPP excited by a limited narrow Bessel beam. It is shown that outside the region of the exciting source the Bessel SPP decays exponentially in the radial direction. It is established that the 1/𝑒 energy-attenuation radius of Bessel SPP, generated by the limited narrow Bessel beam, coincides with the decay length of the propagating surface plasmon.

We have analyzed the cases of symmetric and asymmetric “dielectric-metal-dielectric” structures. A dispersion equation has been derived and numerically analyzed for these cases. The possibility is shown of excitation of two types (low- and high-index) of Bessel surface plasmon polaritons characterized by various profiles of longitudinal component 𝐸^𝑙(𝑧) of electric vector inside the metal film. It has been established that in a symmetric “dielectric-metal-dielectric” structure, the profile of 𝐸^𝑙(𝑧) for low-index Bessel surface plasmon polaritons turns out to be a symmetric relatively medium plane of the metal film. For high-index Bessel surface plasmon polariton mode it is antisymmetric. In an asymmetric “dielectric-metal-dielectric” structure, the distribution of 𝐸^𝑙(𝑧) inside metal film losses symmetry with respect to the medium plane of the metal layer for both generated plasmon polaritons. Moreover, there is a definite value 𝑧_𝑒 of the longitudinal coordinate inside the layer, for which the longitudinal component of the electric vector 𝐸^𝑙 for high-index Bessel SPP is equal to zero. It is shown that if the difference between the refraction indices of adjoining dielectrics and a metal layer decreases, the position 𝑧_𝑒 shifts toward the medium plane of metal film.

The dependence has been investigated of conditions of excitation of Bessel surface plasmon polaritons on the metal layer thickness ℎ. It has been shown that if ℎ increases, the degeneration of Bessel plasmon modes occur. Here, the Bessel surface plasmon polariton mode effective index approaches the one for the case of excitation of Bessel SPP at the boundary of two semi-infinite media, that is, dielectric and metal.

The intensity distribution of low- and high-index Bessel surface plasmon polaritons inside and outside the metal layer have been calculated and analyzed. A two- and three-dimensional pattern of the intensity for the single Bessel SPPs as well as for a superposition of two Bessel SPPs with opposite topological charges has been calculated. It is shown that while increasing the distance from the surface of the metal layer, the central peak of Bessel SPP generated in the structure decays exponentially, but its transversal size does not change.

It is established that the plasmon polariton field, excited by the superposition of two Bessel beams with opposite topological charges, is characterized by the azimuthal modulation of intensity. Owing to it, the intensity pattern is separated into substructures of a nanoscale transverse size. It is shown that the above-mentioned substructures are rather stable when moving off the interface. Thus, using the superposition of two opposite charged vortex Bessel SPPs, which keeps their transversal size at any distance ranging from zero up to about the wavelength, one can form near the interface an array of diffraction-free nanoscale light “needles.” This field is associated with creating a Bessel surface plasmon polariton multitip which is perspective for probing the surface simultaneously through several channels. An experimental set-up is proposed for producing such a Bessel surface plasmon polariton multitip.

The results obtained can be used for the development and optimization of techniques and devices for testing the quality of the surface of various substrates by Bessel surface plasmon polaritons; for creating Bessel surface plasmon polariton-based optical tweezing systems; and for the capturing and manipulating of nanoparticles; applications are expected to be found in near-field optical microscopy with a nanoscale resolution.